Citation: Alain Miranville. The Cahn–Hilliard equation and some of its variants[J]. AIMS Mathematics, 2017, 2(3): 479-544. doi: 10.3934/Math.2017.2.479
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The Cahn–Hilliard system
{∂u∂t=κΔμ, κ>0,μ=−αΔu+f(u), α>0, | (1.1) |
and, equivalently, the Cahn–Hilliard equation
∂u∂t+ακΔ2u−κΔf(u)=0 | (1.2) |
play an essential role in materials science as they describe important qualitative features of two-phase systems related with phase separation processes, assuming isotropy and a constant temperature. This can be observed, e.g., when a binary alloy is cooled down sufficiently. One then observes a partial nucleation (i.e., the apparition of nuclides in the material) or a total nucleation, known as spinodal decomposition: the material quickly becomes inhomogeneous, resulting in a very finely dispersed microstructure. In a second stage, which is called coarsening, occurs at a slower time scale and is less understood, these microstructures coarsen. Such phenomena play an essential role in the mechanical properties of the material, e.g., strength, hardness, fracture toughness and ductility. We refer the reader to, e.g., [58,60,255,259,276,277,311,313] for more details.
Here, u is the order parameter (one usually considers a rescaled density of atoms or concentration of one of the material's components which takes values between −1 and 1, −1 and 1 corresponding to the pure states; the density of the second component is 1−u, meaning that the total density is a conserved quantity) and μ is the chemical potential. Furthermore, f is the derivative of a double-well potential F whose wells correspond to the phases of the material. A thermodynamically relevant potential F is the following logarithmic function which follows from a mean-field model:
F(s)=θc2(1−s2)+θ2[(1−s)ln(1−s2)+(1+s)ln(1+s2)], s∈(−1,1), 0<θ<θc, | (1.3) |
i.e.,
f(s)=−θcs+θ2ln1+s1−s, | (1.4) |
although such a function is very often approximated by regular ones, typically, F(s)=14(s2−1)2, i.e., f(s)=s3−s; more generally, one can take F(s)=14(s2−β2)2, β∈R. The logarithmic terms in (1.3) correspond to the entropy of mixing and θ and θc are proportional to the absolute temperature (assumed constant during the process) and a critical temperature, respectively; the condition θ<θc ensures that F has indeed a double-well form and that phase separation can occur. Also note that the polynomial approximation is reasonable when the quench is shallow, i.e., when the absolute temperature is close to the critical one. Finally, κ is the mobility and α is related to the surface tension at the interface.
We assume in this article that the mobility is a strictly positive constant. Actually, κ is often expected to depend on the order parameter and to degenerate at the singular points of f in the case of a logarithmic nonlinear term (see [59,138,139,178,370]; see also [373] for a discussion in the context of immiscible binary fluids). Note however that this essentially restricts the diffusion process to the interfacial region and is observed, typically, when the movements of atoms are confined to this region (see [330]). In that case, the first equation of (1.1) reads
∂u∂t=div(κ(u)∇μ), |
where, typically, κ(s)=1−s2. In particular, the existence of solutions to the Cahn–Hilliard equation with degenerate mobilities and logarithmic nonlinearities is proved in [138]. The asymptotic behavior, and, more precisely, the existence of attractors, of the Cahn–Hilliard equation with nonconstant mobilities is studied in [342,343].
From a phenomenological point of view, the Cahn–Hilliard system can be derived as follows. One considers the following (total) free energy, called Ginzburg–Landau free energy:
ΨΩ(u,∇u)=∫Ω(α2|∇u|2+F(u))dx, | (1.5) |
where |⋅| denotes the usual Euclidean norm and Ω⊂Rn, n=1, 2 or 3, is the domain occupied by the material.
We can note that the gradient term in the Ginzburg–Landau free energy accounts for the fact that the interactions between the material's components are assumed to be short-ranged. Actually, this term is obtained by approximation of a nonlocal term which also accounts for long-ranged interactions (see [60]). The Cahn–Hilliard equation, with a nonlocal term, was derived rigorously by G. Giacomin and J.L. Lebowitz in [188,189], based on stochastic arguments, by considering a lattice gas with long range Kac potentials (i.e., the interaction energy between two particles at x and y (x, y∈Zn) is given by γnK(γ|x−y|), γ>0 being sent to 0 and K being a smooth function). In that case, the (total) free energy reads
ΨΩ(u)=∫Tn[f(u(x))+u(x)∫TnK(|x−y|)(1−u(y))dy]dx, | (1.8) |
where Tn is the n-dimensional torus. Furthermore, rewriting the total free energy in the form
ΨΩ(u)=∫Tn[f(u(x))+k1(x)u(x)(1−u(x))+12∫TnK(|x−y|)|u(x)−u(y)|2dy]dx, |
where k1(x)=∫TnK(|x−y|)dy, one can, by expanding the last term and keeping only some terms in the expansion, recover the Ginzburg–Landau free energy (this is reasonable when the scale on which the free energy varies is large compared with γ−1; the macroscopic evolution is observed here on the spatial scale γ−1 and time scale γ−2). Such models were studied, e.g., in [2,23,162,168] (see also [72,216,217,218] for the numerical analysis and simulations).
One then has the mass balance
∂u∂t=−divh, | (1.6) |
where h is the mass flux which is related to the chemical potential μ by the following (postulated) constitutive equation which resembles the Fick's law:
h=−κ∇μ. | (1.7) |
The usual definition of the chemical potential is that it is the derivative of the free energy with respect to the order parameter. Here, such a definition is incompatible with the presence of ∇u in the free energy. Instead, μ is defined as a variational derivative of the free energy with respect to u, which yields (assuming proper boundary conditions)
μ=−αΔu+f(u), | (1.8) |
whence the Cahn–Hilliard system.
The Cahn–Hilliard system/equation is now well understood, at least from a mathematical point of view. In particular, one has a rather complete picture as far as the existence, the uniqueness and the regularity of solutions and the asymptotic behavior of the associated dynamical system are concerned. We refer the reader to (among a huge literature), e.g., [4,31,53,88,91,116,123,132,134,138,140,143,163,164,172,245,258,264,274,301,302,305,307,308,309,310,311,313,326, 329,335,349,368,376]. As far as the asymptotic behavior of the system is concerned, one has, in particular, the existence of finite-dimensional attractors. Such sets give information on the global/ all possible dynamics of the system. Furthermore, the finite dimensionality means, very roughly speaking, that, even though the initial phase space is infinite-dimensional, the limit dynamics can be described by a finite number of parameters. We refer the interested reader to, e.g., [15,92,125,303,349] for more details and discussions on this. One also has the convergence of single trajectories to steady states.
Now, it is interesting to note that the Cahn–Hilliard equation and some of its variants are also relevant in other phenomena than phase separation in binary alloys. We can mention, for instance, dealloying (this can be observed in corrosion processes, see [145]), population dynamics (see [95]), tumor growth (see [14,244]), bacterial films (see [253]), thin films (see [315,350]), chemistry (see [354]), image processing (see [24,25,66,73,124]) and even the rings of Saturn (see [353]) and the clustering of mussels (see [271]).
In particular, several such phenomena can be modeled by the following generalized Cahn–Hilliard equation:
∂u∂t+ακΔ2u−κΔf(u)+g(x,u)=0, α, κ>0 | (1.9) |
(here, α and κ do not necessarily have the same physical meaning as in the original Cahn–Hilliard equation). The above general equation contains, in particular, the following models:
(ⅰ) Mixed Allen–Cahn/Cahn–Hilliard system. In that case, we consider the following system of equations:
{∂u∂t=ε2DΔμ−μ, D, ε>0,μ=−Δu+f(u)ε2, |
which can be rewritten, equivalently, as
∂u∂t+ε2DΔ2u−Δ(Df(u)+u)+f(u)ε2=0 |
and is indeed of the form above. In particular, without the term ε2DΔμ in the first equation, we have the Allen–Cahn equation and, without the term −μ, we have the Cahn–Hilliard equation. These equations were proposed in order to account for microscopic mechanisms such as surface diffusion and adsorption/desorption (see [238,240,241,281]) and were studied in [232,233,234,235,239].
(ⅱ) Cahn–Hilliard–Oono equation (see [287,314,355]). In that case,
g(x,s)=g(s)=βs, β>0. |
This function was proposed in [314] in order to account for long-ranged (i.e., nonlocal) interactions in phase separation, but also to simplify numerical simulations, due to the fact that we do not have to account for the conservation of mass (see below), although it seems that this equation has never been considered in simulations. A variant of this model, proposed in [90] to model microphase separation of diblock copolymers, consists in taking
g(x,s)=g(s)=β(s−1Vol(Ω)∫Ωu0(x)dx), β>0, |
where u0 is the initial condition. In that case, we have the conservation of mass and efficient simulations, based on multigrid solvers, were performed in [13]. This variant of the Cahn–Hilliard–Oono equation can also be coupled with the incompressible Navier–Stokes equations to model a chemically reacting binary fluid (see [228,229]; see also [43] for the mathematical analysis).
(ⅲ) Proliferation term. In that case,
g(x,s)=g(s)=λs(s−1), λ>0. |
This function was proposed in [244] in view of biological applications and, more precisely, to model wound healing and tumor growth (in one space dimension) and the clustering of brain tumor cells (in two space dimensions); see also [354] for other quadratic functions with chemical applications and [14] for other polynomials with biological applications.
(ⅳ) Fidelity term. In that case,
g(x,s)=λ0χΩ∖D(x)(s−h(x)), λ0>0, D⊂Ω, h∈L2(Ω), |
where χ denotes the indicator function, and we consider the following equation:
∂u∂t+εΔ2u−1εΔf(u)+g(x,u)=0, ε>0. |
Written in this way, ε corresponds to the interface thickness. This function g was proposed in [24,25] in view of applications to image inpainting. Here, h is a given (damaged) image and D is the inpainting (i.e., damaged) region. Furthermore, the fidelity term g(x,u) is added in order to keep the solution close to the image outside the inpainting region. The idea in this model is to solve the equation up to steady state to obtain an inpainted (i.e., restored) version u(x) of h(x).
The generalized equation (1.9) was studied in [288,292] (see also [148]) under very general assumptions on the additional term g, when endowed with Dirichlet boundary conditions. In that case, one essentially recovers the results (well-posedness, regularity and existence of finite-dimensional attractors) known for the original Cahn–Hilliard equation. The case of Neumann boundary conditions is much more involved, due to the fact that one no longer has the conservation of mass, i.e., of the spatial average of the order parameter, when compared with the original Cahn–Hilliard equation with Neumann boundary conditions (see [73,74,85,148,149]).
Another variant of the Cahn–Hilliard equation, which we will not address in this review, is concerned with higher-order Cahn–Hilliard models. More precisely, G. Caginalp and E. Esenturk recently proposed in [57] (see also [70]) higher-order phase-field models in order to account for anisotropic interfaces (see also [254,348,363] for other approaches which, however, do not provide an explicit way to compute the anisotropy). More precisely, these authors proposed the following modified free energy, in which we omit the temperature:
ΨHOGL=∫Ω(12∑Mi=1∑|k|=iak|Dku|2+F(u))dx, M∈N, | (1.10) |
where, for k=(k1,k2,k3)∈(N∪{0})3,
|k|=k1+k2+k3 |
and, for k≠(0,0,0),
Dk=∂|k|∂xk11∂xk22∂xk33 |
(we agree that D(0,0,0)v=v). The corresponding higher-order Cahn–Hilliard equation then reads
∂u∂t−Δ∑Mi=1(−1)i∑|k|=iakD2ku−Δf(u)=0. | (1.11) |
For M=1 (anisotropic Cahn–Hilliard equation), we have an equation of the form
∂u∂t+Δ∑3i=1ai∂2u∂x2i−Δf(u)=0 |
and, for M=2 (sixth-order anisotropic Cahn–Hilliard equation), we have an equation of the form
∂u∂t−Δ∑3i,j=1aij∂4u∂x2i∂x2j+Δ∑3i=1bi∂2u∂x2i−Δf(u)=0. |
We studied in [81] the corresponding higher-order isotropic model, namely,
∂u∂t−ΔP(−Δ)u−Δf(u)=0, | (1.12) |
where
P(s)=∑Mi=1aisi, ak>0, M≥1, s∈R, |
and, in [82], the anisotropic higher-order model (1.11) (there, numerical simulations were also performed to illustrate the effects of the higher-order terms and of the anisotropy). Furthermore, these models contain sixth-order Cahn–Hilliard models. We can note that there is currently a strong interest in the study of sixth-order Cahn–Hilliard equations. Such equations arise in situations such as strong anisotropy effects being taken into account in phase separation processes (see [352]), atomistic models of crystal growth (see [24,25,144,173]), the description of growing crystalline surfaces with small slopes which undergo faceting (see [341]), oil-water-surfactant mixtures (see [200,201]) and mixtures of polymer molecules (see [115]). We refer the reader to [68,208,213,214,215,227,256,257,278,279,287,289,290,291,293,316,317,322,323,356,357,367] for the mathematical and numerical analysis of such models.
We can also note that the variant (1.9) can be relevant in the context of higher-order models (we can mention, for instance, anisotropic effects in tumor growth). We refer the reader to [83] for the analysis and numerical simulations of such models.
Our aim in this article is to review and discuss some of the aforementioned Cahn–Hilliard models (1.9). More precisely, we will focus on the last three examples mentioned above. We also discuss the original Cahn–Hilliard equation, with an emphasis on the thermodynamically relevant logarithmic nonlinear terms.
The Cahn–Hilliard system, in a bounded and regular domain Ω of Rn, n=1, 2 or 3, usually is endowed with Neumann boundary conditions, namely,
∂μ∂ν=0, on Γ, | (2.1) |
meaning that there is no mass flux at the boundary (note that h.ν=−κ∂μ∂ν), and
∂u∂ν=0, on Γ, | (2.2) |
which is a natural variational boundary condition (it also yields that the interface is orthogonal to the boundary). Here, Γ=∂Ω and ν is the unit outer normal to the boundary. In particular, it follows from the first boundary condition that we have the conservation of mass, i.e., of the spatial average of the order parameter, obtained by (formally) integrating the first equation of (1.1) over Ω,
⟨u(t)⟩=1Vol(Ω)∫Ωu(t,x)dx=⟨u(0)⟩, ∀t≥0. | (2.3) |
If we have in mind the fourth-order in space Cahn–Hilliard equation, we can rewrite these boundary conditions, equivalently, as
∂u∂ν=∂Δu∂ν=0, on Γ. | (2.4) |
Remark 2.1. We can also consider periodic boundary conditions (in which case Ω=Πni=1(0,Li), Li>0, i=1,\..., n).
As mentioned in the introduction, the Cahn–Hilliard equation is now well understood from a mathematical point of view. This is in particular the case for the usual cubic nonlinear term f(s)=s3−s, but also for more general regular nonlinear terms.
Now, the case of the thermodynamically relevant logarithmic nonlinear terms is more difficult. Indeed, in order to prove the existence of a solution, one generally approximates the singular nonlinear term by regular ones (e.g., by polynomials as in [116]; we also mention [4,301] for different approaches, based on semigroup theory and a regularization by the viscous Cahn–Hilliard equation proposed in [310], respectively) and one then passes to the limit. But then, when passing to the limit, one must make sure that the order parameter stays in the physically relevant interval ((−1,1) in our case); otherwise the equations would not make sense. From a physical point of view, this separation property says that, in the phase separation process, one never completely reaches the pure states.
Remark 2.2. It would be interesting to see whether, for a regular nonlinear term and, in particular, for the usual cubic one, the order parameter also remains in the physically relevant interval. This is however not the case and one can construct simple counterexamples, already in one space dimension (see [324]).
We now give a proof of existence of a solution which is based on proper approximations of the logarithmic nonlinear term and which can be easily extended to more general singular nonlinear terms (see also [140]).
We actually consider the following more general initial and boundary value problem:
∂u∂t+βu=Δμ, β≥0, | (2.5) |
μ=−Δu+f(u), | (2.6) |
∂u∂ν=∂μ∂ν=0, on Γ, | (2.7) |
u|t=0=u0. | (2.8) |
When β=0, we recover the original Cahn–Hilliard equation, and, when β>0, we have the Cahn–Hilliard–Oono equation (here, we have set the other parameters equal to 1).
Remark 2.3. (ⅰ) As mentioned in the introduction, the term βu, β>0, models nonlocal interactions. In particular, short-ranged interactions tend to homogenize the system, whereas long-ranged ones forbid the formation of too large structures; the competition between these two effects translates into the formation of a micro-separated state (also called super-crystal) with a spatially modulated order parameter, defining structures with a uniform size (see [355] for more details and references).
(ⅱ) Actually, it can be surprising that nonlocal interactions can be described by such a simple linear term. This can be seen by noting that the equations are obtained by considering the free energy
ψ=|∇u|2+F(u)+∫Ωu(y)g(y,x)u(x)dy, | (2.9) |
where the function g describes the long-ranged interactions. In particular, in Oono's model and, e.g., in three space dimensions, one takes
g(y,x)=4πβ|y−x|, β>0. | (2.10) |
Note that the long-ranged interactions are repulsive when u(y) and u(x) have opposite signs and thus favor the formation of interfaces (see [355] and the references therein). We finally write, as in the derivation of the classical Cahn–Hilliard equation,
∂u∂t=∂uψ, | (2.11) |
where ∂u denotes the variational derivative with respect to u. Noting that −1|y−x| is the Green function associated with the Laplace operator and defining μ as above, we obtain (2.5)-(2.6) (see [355] and the references therein for more details).
Remark 2.4. It is easier to prove the existence of a weak solution to the Cahn–Hilliard system with the degenerate mobility κ(s)=1−s2 and the thermodynamically relevant logarithmic nonlinear term (1.4). Indeed, one uses the fact that κ(s)f′(s) is bounded (see [138] for details). Here, we can adapt the techniques in [138] to the Cahn–Hilliard–Oono equation.
As far as the nonlinear term f is concerned, we assume more generally that
f∈C1(−1,1), f(0)=0, | (2.12) |
lims→±1f(s)=±∞, lims→±1f′(s)=+∞. | (2.13) |
In particular, it follows from these assumptions that
f′≥−c0, c0≥0, | (2.14) |
−c1≤F(s)≤f(s)s+c2, c1, c2≥0, s∈(−1,1), | (2.15) |
where F(s)=∫s0f(r)dr (in particular, in order to obtain the second of (2.15), we can study the variations of the function s↦f(s)s−F(s)+c02s2, whose derivative has, owing to (2.14), the sign of s).
Remark 2.5. In particular, the thermodynamically relevant logarithmic functions (1.4) satisfy the above assumptions.
Next, we define, for N∈N, the approximated functions fN∈C1(R) by
fN(s)={f(−1+1N)+f′(−1+1N)(s+1−1N), s<−1+1N,f(s), |s|≤1−1N,f(1−1N)+f′(1−1N)(s−1+1N), s>1−1N. |
We thus have
f′N≥−c0 | (2.16) |
and, setting FN(s)=∫s0fN(r)dr,
−c3≤FN(s)≤c4fN(s)s+c5, c4>0, c3, c5≥0, s∈R, | (2.17) |
fN(s)s≥c6|fN(s)|−c7, c6>0, c7≥0, | (2.18) |
where the constants ci, i=3, ..., 7, are independent of N (see [305]). Actually, there holds, more generally, for N large enough (see [301], Proposition A.1, and [305] for details),
fN(s+m)s≥c′m(|fN(s+m)|+FN(s+m))−c″m, | (2.19) |
c′m>0, c″m≥0, s∈R, m∈(−1,1), |
where the constants c′m and c″m are independent of N and depend continuously and boundedly on m.
We finally introduce the approximated problems
∂uN∂t+βuN=ΔμN, | (2.20) |
μN=−ΔuN+fN(uN), | (2.21) |
∂uN∂ν=∂μN∂ν=0, on Γ, | (2.22) |
uN|t=0=u0. | (2.23) |
We denote by ((⋅,⋅)) the usual L2-scalar product, with associated norm ‖⋅‖. We further set ‖⋅‖−1=‖(−Δ)−12⋅‖, where (−Δ)−1 denotes the inverse minus Laplace operator associated with Neumann boundary conditions and acting on functions with null spatial average. More generally, ‖⋅‖X denotes the norm on the Banach space X.
We set, for v∈L1(Ω),
⟨v⟩=1Vol(Ω)∫Ωvdx, |
and, for v∈H1(Ω)′,
⟨v⟩=1Vol(Ω)⟨v,1⟩H1(Ω)′,H1(Ω). |
We note that
v↦(‖v−⟨v⟩‖2−1+⟨v⟩2)12 |
is a norm on H1(Ω)′ which is equivalent to the usual norm. Similarly,
v↦(‖v−⟨v⟩‖2+⟨v⟩2)12 |
and
v↦(‖∇v‖2+⟨v⟩2)12 |
are norms on L2(Ω) and H1(Ω), respectively, which are equivalent to their usual norms.
We further set
W={v∈H1(Ω), ⟨v⟩=0} |
and note that, on W, the generalized Poincaré's inequality
‖v‖≤c‖∇v‖ |
holds. Moreover, we have the continuous embedding H−1(Ω)⊂W′.
In what follows, the same letters c, c′ and c″ denote (generally positive) constants which may vary from line to line and which are independent of N.
Our aim in this subsection is to derive a priori estimates for the solutions uN and μN to (2.20)-(2.23). These a priori estimates are independent of N and are formal, i.e., we assume that uN and μN are as smooth as needed. The crucial step, to prove the existence of a solution, consists in deriving an a priori estimate independent of N on fN(uN) in L2((0,T)×Ω), T>0.
Classically, these a priori estimates allow us to obtain the existence of a solution to (2.20)-(2.23) by implementation of a Galerkin approximation (see, e.g., [287] for more details). This will also allow us to pass to the limit N→+∞ in the approximated system (2.20)-(2.23).
From now on, we assume that
‖u0‖L∞(Ω)≤1−δ, δ∈(0,1), | (2.24) |
where δ is a fixed constant.
First, integrating (2.20) over Ω, we find
d⟨uN⟩dt+β⟨uN⟩=0, | (2.25) |
which yields
⟨uN(t)⟩=e−βt⟨u0⟩, t≥0. | (2.26) |
We thus deduce from (2.26) that
|⟨uN(t)⟩|≤|⟨u0⟩|, t≥0, | (2.27) |
whence, in view of (2.24),
|⟨uN(t)⟩|≤1−δ, t≥0, | (2.28) |
i.e., ⟨uN⟩ is strictly separated from the pure states ±1.
Then, setting, for a function φ defined in Ω, ¯φ=φ−⟨φ⟩, we can rewrite (2.20) in the equivalent form
∂¯uN∂t+β¯uN=ΔμN, | (2.29) |
μN=−Δ¯uN+fN(uN), | (2.30) |
owing to (2.25).
In a next step, we multiply (2.29) by μN. Integrating over Ω and by parts, we obtain
‖∇μN‖2+((∂¯uN∂t,μN))+β((¯uN,μN))=0. | (2.31) |
Furthermore, it follows from (2.30) that
((∂¯uN∂t,μN))+β((¯uN,μN))=12ddt‖∇¯uN‖2+ddt∫ΩFN(uN)dx | (2.32) |
−((d⟨uN⟩dt,fN(uN)))+β‖∇¯uN‖2+β((¯uN,fN(uN))). |
Noting that it follows from (2.25) that
−((d⟨uN⟩dt,fN(uN)))=β((⟨uN⟩,fN(uN))), | (2.33) |
we finally deduce from (2.18) and (2.31)-(2.33) the differential inequality
ddt(‖∇¯uN‖2+2∫ΩFN(uN)dx) | (2.34) |
+c(‖∇¯uN‖2+‖fN(uN)‖L1(Ω)+‖∇μN‖2)≤c′, c>0. |
We then multiply (2.30) by ¯uN and find, owing to (2.19) (taking s=¯uN and m=⟨uN⟩) and to the Poincaré inequality on W,
‖∇¯uN‖2+c(‖fN(uN)‖L1(Ω)+∫ΩFN(uN)dx)≤c′+((μN,¯uN))=c′+((¯μN,¯uN)) |
≤c′+c″‖∇¯uN‖‖∇μN‖, |
where the constants c, c′ and c″ depend on δ, but are independent of N, at least for N large enough, whence
‖∇¯uN‖2+c(‖fN(uN)‖L1(Ω)+∫ΩFN(uN)dx)≤c′+c″‖∇μN‖2, c>0. | (2.35) |
Summing (2.34) and ξ1 times (2.35), where ξ1>0 is small enough, we have the differential inequality
dENdt+c(EN+‖fN(uN)‖L1(Ω)+‖∇μN‖2)≤c′, c>0, | (2.36) |
where
EN=‖uN‖2+‖∇¯uN‖2+2∫ΩFN(uN)dx. | (2.37) |
We now rewrite (2.29) in the equivalent form
(−Δ)−1∂¯uN∂t+β(−Δ)−1¯uN=−¯μN | (2.38) |
(note indeed that ⟨∂¯uN∂t⟩=0). Multiplying (2.38) by ∂¯uN∂t, we obtain
β2ddt‖¯uN‖2−1+‖∂¯uN∂t‖2−1=−((¯μN,∂¯uN∂t)). | (2.39) |
We note that, thanks to the Poincaré inequality on W,
|((¯μN,∂¯uN∂t))|≤c‖∂¯uN∂t‖−1‖∇μN‖ | (2.40) |
≤14‖∂¯uN∂t‖2−1+c‖∇μN‖2. |
It thus follows from (2.39) that
βddt‖¯uN‖2−1+‖∂¯uN∂t‖2−1≤c‖∇μN‖2. | (2.41) |
Next, we note that it follows from (2.30) that
¯μN=−Δ¯uN+¯fN(uN). | (2.42) |
Multiplying (2.42) by −Δ¯uN, we find, owing to (2.16),
‖Δ¯uN‖2≤c0‖∇¯uN‖2−((¯μN,Δ¯uN)) |
≤c0‖∇¯uN‖2+12‖Δ¯uN‖2+c‖∇μN‖2, |
which yields
‖Δ¯uN‖2≤2c0‖∇¯uN‖2+c‖∇μN‖2. | (2.43) |
Summing (2.36) and ξ2 times (2.43), where ξ2>0 is small enough, we have the differential inequality
dENdt+c(EN+‖¯uN‖2H2(Ω)+‖fN(uN)‖L1(Ω)+‖∇μN‖2)≤c′, c>0. | (2.44) |
We also note that (2.42) implies
‖¯fN(uN)‖≤c(‖¯uN‖H2(Ω)+‖∇μN‖), | (2.45) |
which, combined with (2.44), yields
dENdt+c(EN+‖¯uN‖2H2(Ω)+‖fN(uN)‖L1(Ω)+‖¯fN(uN)‖2+‖∇μN‖2) | (2.46) |
≤c′, c>0. |
Finally, taking s=¯uN and m=⟨uN⟩ in (2.19) and integrating over Ω, we obtain, owing to (2.28),
∫Ω|fN(uN)|dx≤c|∫ΩfN(uN)¯uNdx|+c′, |
where the constants c and c′ only depend on δ (and are, in particular, independent of N), so that
|⟨fN(uN)⟩|≤c|∫Ω¯fN(uN)¯uNdx|+c′ |
and
|⟨fN(uN)⟩|≤c‖¯uN‖‖¯fN(uN)‖+c′. | (2.47) |
Since
‖fN(u)‖2≤c(‖¯fN(uN)‖2+|⟨fN(uN)⟩|2), |
it follows from (2.47) that
‖fN(uN)‖L2((0,T)×Ω) | (2.48) |
≤c(‖¯fN(uN)‖L2((0,T)×Ω)+‖¯uN‖L∞(0,T;L2(Ω))‖¯fN(uN)‖L2((0,T)×Ω))+c′, T>0. |
Now, Poincaré's inequality and (2.46) imply that
‖¯fN(uN)‖2L2((0,T)×Ω)≤cEN(0)+c′T |
and
‖¯uN‖2L∞(0,T;L2(Ω))≤c‖∇¯uN‖2L∞(0,T;L2(Ω)n)≤c′EN(0)+c″T. |
It thus follows from (2.48) that
‖fN(uN)‖L2((0,T)×Ω)≤cT,δ(‖u0‖2H1(Ω)+1), T>0, | (2.49) |
where the constant cT,δ is independent of N, at least for N large enough. Here, we have used the fact that, owing to (2.24), if N is large enough, FN(u0)=F(u0), so that we can handle the term ∫ΩFN(u0)dx which appears in the right-hand side when integrating (2.46) with respect to time.
We also note that (2.46) and Gronwall's lemma imply the dissipative estimate
EN(t)≤e−ctEN(0)+c′, c>0, t≥0, | (2.50) |
which yields
‖uN(t)‖H1(Ω)≤cδe−c′t(‖u0‖H1(Ω)+1)+c″, c′>0, t≥0. | (2.51) |
Finally, noting that ⟨μN⟩=⟨fN(uN)⟩, it follows from (2.46) and (2.49) that
‖μN‖L2(0,T;H1(Ω))≤cT,δ(‖u0‖2H1(Ω)+1), T>0. | (2.52) |
We have the
Theorem 2.6. We assume that u0 is given such that u0∈H1(Ω) and ‖u0‖L∞(Ω)<1. Then, (2.5)-(2.8) possesses at least one (weak) solution such that, ∀T>0,
u∈C([0,T];H1(Ω)w)∩L2(0,T;H2(Ω)), |
∂u∂t∈L2(0,T;H1(Ω)′), |
μ∈L2(0,T;H1(Ω)), |
where the subscript w stands for the weak topology, and
ddt((u,q))+β((u,q))=−((∇μ,∇q)), |
((μ,Ξ))=((∇u,∇Ξ))+((f(u),Ξ)), |
a.e. t∈[0,T], ∀q, Ξ∈C∞c(Ω),
u(0)=u0. |
Furthermore, u∈C([0,T];H1−η(Ω)), ∀η>0, and −1<u(t,x)<1, a.e. (t,x).
Proof. We consider a solution (uN,μN) to the approximated problem (2.20)-(2.23) (the proof of existence of such a solution having the above regularity can be obtained by a standard Galerkin scheme).
Furthermore, since the estimates derived in the previous section are independent of N, this solution converges, up to a subsequence which we do not relabel, to a limit function (u,μ) in the following sense:
uN→u in L∞(0,T;H1(Ω)) weak star and in L2(0,T;H2(Ω)) weakly, |
∂uN∂t→∂u∂t in L2(0,T;H1(Ω)′) weakly, |
uN→u a.e. (t,x) and in L2((0,T)×Ω), |
μN→μ in L2(0,T;H1(Ω)) weakly. |
Here, we have used (2.41), (2.51)-(2.52) and classical Aubin–Lions compactness results.
The only difficulty, when passing to the limit, is to pass to the limit in the nonlinear term fN(uN).
First, it follows from (2.46) that fN(uN) is bounded, independently of N, in L1((0,T)×Ω). Then, it follows from the explicit expression of fN that
meas(EN,M)≤φ(1N), N≤M, |
where
EN,M={(t,x)∈(0,T)×Ω, |uM(t,x)|>1−1N} |
and
φ(s)=cmax(|f(1−s)|,|f(s−1)|). |
Here, the constant c is independent of N and M. Note indeed that there holds
∫T0∫Ω|fM(uM)|dxdt≥∫EN,M|fM(uM)|dxdt≥c′meas(EN,M)1φ(1N), | (2.53) |
where the constant c′ is independent of N and M. We can pass to the limit M→+∞ (employing Fatou's lemma, see (2.53)) and then N→+∞ (noting that lims→0φ(s)=0) to find
meas{(t,x)∈(0,T)×Ω, |u(t,x)|≥1}=0, |
so that
−1<u(t,x)<1, a.e. (t,x). | (2.54) |
Next, it follows from the above almost everywhere convergence of uN to u, from (2.54) and the explicit expression of fN that
fN(uN)→f(u), a.e. (t,x)∈(0,T)×Ω. | (2.55) |
Finally, since, owing to (2.49), fN(uN) is bounded, independently of N, in L2((0,T)×Ω), it follows from (2.55) that fN(uN)→f(u) in L2((0,T)×Ω) weakly, which finishes the proof of the passage to the limit.
Remark 2.7. We consider the particular case of the physically relevant nonlinear term (1.4). In that case, it is not difficult to see that the function F(s)=∫s0f(r)dr is bounded on (−1,1). Noting then that the function FN(s)=∫s0fN(r)dr is given by
FN(s)={F(−1+1N)+f(−1+1N)(s+1−1N)+12f′(−1+1N)(s+1−1N)2, s<−1+1N,F(s), |s|≤1−1N,F(1−1N)+f(1−1N)(s−1+1N)+12f′(1−1N)(s−1+1N)2, s>1−1N, |
elementary computations show that FN is also bounded on (−1,1). Therefore, we can relax the assumptions of Theorem 2.6 and assume that u0 only satisfies −1<u0(x)<1, a.e. x∈Ω, and |⟨u0⟩|<1. Indeed, we deduce from the above that ∫ΩFN(u0)dx is bounded independently of N and we do not need the strict separation property (2.24) to derive the a priori estimates on uN, namely, when integrating (2.46) with respect to time.
Remark 2.8. (ⅰ) It is not difficult to prove the uniqueness of solutions. Indeed, let u1 and u2 be two solutions with initial conditions u10 and u20, respectively, such that ⟨u10⟩=⟨u20⟩. Then, we have, setting u=u1−u2 and u0=u10−u20 and noting that ⟨u⟩=0,
(−Δ)−1∂u∂t+β(−Δ)−1u−Δu+f(u1)−f(u2)−⟨f(u1)−f(u2)⟩=0, | (2.56) |
∂u∂ν=0, on Γ, | (2.57) |
u|t=0=u0. | (2.58) |
Multiplying (2.56) by u, we obtain, in view of (2.14),
12ddt‖u‖2−1+β‖u‖2−1+‖∇u‖2≤c0‖u‖2. | (2.59) |
Employing the interpolation inequality
‖u‖2≤c‖u‖−1‖∇u‖, | (2.60) |
we deduce that
ddt‖u‖2−1+c‖u‖2H1(Ω)≤c′‖u‖2−1, c>0. | (2.61) |
It follows from (2.61) and Gronwall's lemma that
‖u(t)‖H−1(Ω)≤cec′t‖u0‖H−1(Ω), t≥0, | (2.62) |
whence the continuous dependence with respect to the initial conditions (in the H−1-norm) and the uniqueness (for u; the uniqueness for μ is then straightforward).
(ⅱ)) We set
Φm={v∈H1(Ω)∩L∞(Ω), −1<v(x)<1, a.e. x∈Ω, ⟨v⟩=m}, m∈(−1,1). |
It follows from the above that we can define the continuous (for the H−1-norm) family of solving operators
S(t):Φm∩{v∈L∞(Ω), ‖v‖L∞(Ω)<1}→Φm, u0↦u(t), t≥0. |
Furthermore, it follows from (2.51) and Gronwall's lemma that S(t) is dissipative on Φm, i.e., it possesses a bounded absorbing set B0⊂Φm (in the sense that, ∀B⊂Φm bounded, ∃t0=t0(B) such that t≥t0 implies S(t)B⊂B0). Note that, in the case of the thermodynamically relevant logarithmic potentials, the family of solving operators S(t), t≥0, forms a continuous (for the H−1-norm) and dissipative semigroup on Φm. Furthermore, in all cases, it follows from (2.62) that we can extend (in a unique way and by continuity) S(t) to a semigroup acting on the closure of Φm in the H−1-topology, i.e., on Lm={v∈L∞(Ω), ‖v‖L∞(Ω)≤1, ⟨v⟩=m}, meaning that we can now consider initial data which contain the pure states; note that S(t):Lm→Φm, as soon as t>0.
(ⅲ) We can note that the pure states are not (weak) solutions to our problem. However, in [301], we were able to prove, by a careful study of the structure of attractors, that, in the case of the original Cahn–Hilliard equation, the pure states can indeed be considered as weak solutions, by setting S(t)(±1)=±1.
Remark 2.9. We can also study the limit β goes to 0. In particular, we proved in [287] that, for regular nonlinear terms, the asymptotic behavior of the Cahn–Hilliard–Oono equation and the limit Cahn–Hilliard equation are close in some proper sense when β is small. The case of logarithmic nonlinear terms is much more involved and we only proved in [300] the convergence of solutions on finite time intervals.
A natural way to obtain further regularity is to first differentiate the equation for u with respect to time. However, for β>0, such a technique cannot be applied in a direct way and is more involved. Indeed, we recall that we have the equation
(−Δ)−1∂¯uN∂t+β(−Δ)−1¯uN=−¯μN. | (2.63) |
Differentiating (2.63) with respect to time, we have
(−Δ)−1∂∂t∂¯uN∂t+β(−Δ)−1∂¯uN∂t=−∂¯μN∂t, | (2.64) |
where
∂¯μN∂t=−Δ∂¯uN∂t+¯f′N(uN)∂uN∂t. | (2.65) |
Multiplying (2.64) by ∂¯uN∂t, we obtain, owing to (2.65),
12ddt‖∂¯uN∂t‖2−1+β‖∂¯uN∂t‖2−1+‖∇∂¯uN∂t‖2+((f′N(uN)∂uN∂t,∂¯uN∂t))=0. | (2.66) |
We infer from (2.16) that
((f′N(uN)∂uN∂t,∂¯uN∂t))≥−c0‖∂¯uN∂t‖2+((f′N(uN)∂⟨uN⟩∂t,∂¯uN∂t)), |
which yields, owing to a proper interpolation inequality,
ddt‖∂¯uN∂t‖2−1+2β‖∂¯uN∂t‖2−1+‖∇∂¯uN∂t‖2≤c‖∂¯uN∂t‖2−1−2((f′N(uN)∂⟨uN⟩∂t,∂¯uN∂t)). | (2.67) |
The problem is that we now need to estimate the term
((f′N(uN)∂⟨uN⟩∂t,∂¯uN∂t))=−βVol(Ω)⟨uN⟩⟨f′N(uN)∂¯uN∂t⟩ |
(when β=0, this term vanishes) and we are not able to estimate it uniformly with respect to N. Note that, if ⟨u0⟩=0, then ⟨u(t)⟩=0, ∀t≥0, and we do not have this problem.
In order to avoid dealing with this term, we write instead that
((f′N(uN)∂uN∂t,∂¯uN∂t))=((f′N(uN)∂uN∂t,∂uN∂t))−∂⟨uN⟩∂t((f′N(uN)∂uN∂t,1)) |
≥−c0‖∂uN∂t‖2−∂⟨uN⟩∂tddt∫ΩFN(uN)dx |
=−c0‖∂uN∂t‖2−ddt(∂⟨uN⟩∂t∫ΩFN(uN)dx)+∂2⟨uN⟩∂t2∫ΩFN(uN)dx. |
Setting
Λ=12‖∂¯uN∂t‖2−1−∂⟨uN⟩∂t∫ΩFN(uN)dx, |
we infer from (2.66) the differential inequality
dΛdt+β‖∂¯uN∂t‖2−1+‖∇∂¯uN∂t‖2≤c0‖∂uN∂t‖2−∂2⟨uN⟩∂t2∫ΩFN(uN)dx, |
which yields, employing a proper interpolation inequality,
dΛdt+β‖∂¯uN∂t‖2−1+12‖∇∂¯uN∂t‖2≤c(‖∂¯uN∂t‖2−1+|∂⟨uN⟩∂t|2)−∂2⟨uN⟩∂t2∫ΩFN(uN)dx. | (2.68) |
Recalling (2.26) and (2.50), we can see that Λ is bounded from below,
Λ≥12‖∂¯uN∂t‖2−1−c, |
for some positive constant c which is independent of N. Similarly, we can easily prove that the last two terms in the right-hand side of (2.68) are bounded from above. We thus end up with a differential inequality of the form
dΛdt+β‖∂¯uN∂t‖2−1+12‖∇∂¯uN∂t‖2≤c(‖∂¯uN∂t‖2−1+⟨u0⟩2+EN(0)2+1), | (2.69) |
where the positive constant c is independent of N, and we can conclude by using, e.g., the uniform Gronwall's lemma (see, e.g., [349]). We thus see that the additional term βu in the Oono's model brings essential difficulties.
Having this, we can go further and prove additional regularity on uN (see, e.g., [132]). Note however that some corresponding constants may a priori depend on N.
A related question is the strict separation from the pure states, namely, an estimate of the form
‖u(t)‖L∞(Ω)≤1−δ, δ∈(0,1). |
From a physical point of view, this would mean that not only we never have the pure states during the phase separation process, but we also stay in some sense far from the pure states. From a mathematical point of view, this would mean that we actually have the same problem, but with a regular nonlinear term (actually, even better: with a bounded and globally Lipschitz continuous nonlinear term). Studying further regularity on u and the asymptotic behavior of the problem would then be straightforward tasks. This strict separation property is however related with the aforementioned question of the additional regularity; to be more precise, this requires proper estimates on f′(u) (see [301]).
As mentioned above, in [301], one regularizes the Cahn–Hilliard equation by the viscous Cahn–Hilliard equation
ε∂uε∂t+(−Δ)−1∂uε∂t−Δuε+f(uε)−⟨f(uε)⟩=0, ε>0, | (2.70) |
∂uε∂ν=0, on Γ, | (2.71) |
uε|t=0=u0. | (2.72) |
One advantage of the viscous Cahn–Hilliard equation is that one has the strict separation from the pure states. More precisely, one can prove the
Theorem 2.10. We assume that ε>0 and u0∈Dεm, |m|≤1−η, η∈(0,1), where
Dεm={q∈H2(Ω), ∂q∂ν=0, on Γ, ‖q‖L∞(Ω)≤1, ⟨q⟩=m, |
f(q)∈L2(Ω), √εϕ∈L2(Ω), ϕ∈H−1(Ω), ϕ=(εI+(−Δ)−1)−1(Δq−f(q)+⟨f(q)⟩)}. |
Then, for every ξ>0, there holds
‖uε(t)‖L∞(Ω)≤1−δε,η,ξ, ∀t≥ξ, | (2.73) |
where the constant δε,η,ξ∈(0,1) is independent of t and uε. Furthermore, if
‖u0‖L∞(Ω)≤1−δ0, | (2.74) |
for some δ0∈(0,1), then
‖uε(t)‖L∞(Ω)≤1−δ′ε,η,δ0,‖u0‖Dεm, ∀t≥0, | (2.75) |
where
‖q‖2Dεm=‖q‖2H2(Ω)+‖f(q)‖2L2(Ω)+ε‖ϕ‖2L2(Ω)+‖ϕ‖2H−1(Ω) |
and the constant δ′ε,η,δ0,‖u0‖Dεm∈(0,1) is independent of t and uε.
Remark 2.11. It follows from the above that, if ‖u0‖L∞(Ω)≤1, then any solution uε to the viscous Cahn–Hilliard equation is a priori strictly separated from the singularities of f as soon as t>0. Furthermore, if the initial datum is strictly separated from ±1, then uε remains uniformly a priori strictly separated from ±1 for all times.
Remark 2.12. (ⅰ) Unfortunately, both constants δε,η,ξ and δ′ε,η,δ0,‖u0‖Dεm tend a priori to 0+ as ε→0+, so that the above theorem does not say anything on strict separation properties for the solutions to the Cahn–Hilliard equation.
(ⅱ) Actually, we can prove similar strict separation properties for the solutions to the Cahn–Hilliard equation if we further assume that
|f′(s)|≤c(|f(s)|2+1), s∈(−1,1), |
for some positive constant c. In particular, this inequality holds if f has a growth of the form ±1(1−s2)p, p≥1 (we can actually improve this and take p>37, see [301]), close to ±1, but does not hold for the physically relevant logarithmic potentials.
(ⅲ) In one space dimension, owing to the continuous embedding H1(Ω)⊂C(¯Ω), we can easily prove the above strict separation properties for the Cahn–Hilliard equation. Furthermore, in two space dimensions, using the embedding of H1(Ω) into a proper Orlicz space, we can prove these properties, provided that
|f′(s)|≤ec|f(s)|+c′, s∈(−1,1), |
for some positive constants c and c′ (see [301] for details). In particular, the physically relevant logarithmic potentials satisfy these assumptions. Now, in three space dimensions, the strict separation from the singularities is an open problem for the thermodynamically relevant logarithmic nonlinear terms.
An alternative proof, in two space dimensions, based again on the Orlicz embedding and also valid for the Cahn–Hilliard–Oono equation, was given in [192] (see also [119,165,193,195]). There, in order to avoid dealing with the the viscous Cahn–Hilliard equation and differentiating the equation for u with respect to time, we used instead proper truncations and difference quotients. Having the strict separation property (for, say, t≥2 in our case), we can then prove the existence of finite-dimensional attractors and the convergence of single trajectories to steady states.
Remark 2.13. We refer the reader to [129] for the study of the Cahn–Hilliard system with a singular potential in unbounded cylindrical domains (in that case, the equations are endowed with Dirichlet boundary conditions).
The question of how the phase separation process (i.e., the spinodal decomposition) is influenced by the presence of walls has gained much attention (see [155,156,246] and the references therein). This problem has mainly been studied for polymer mixtures (although it should also be important for other systems, such as binary metallic alloys): from a technological point of view, binary polymer mixtures are particularly interesting, since the occurring structures during the phase separation process may be frozen by a rapid quench into the glassy state; microstructures at surfaces on very small length scales can be produced in this way.
We also recall that the usual variational boundary condition ∂u∂ν=0 on the boundary yields that the interface is orthogonal to the boundary, meaning that the contact line, when the interface between the two components meets the walls, is static, which is not reasonable in many situations. This is the case, e.g., for mixtures of two immiscible fluids: in that case, the contact angle should be dynamic, due to the movements of the fluids. This can also be the case in the context of binary alloys, whence the need to define dynamic boundary conditions for the Cahn–Hilliard equation.
In that case, we again write that there is no mass flux at the boundary (i.e., that (2.1) still holds). Then, in order to obtain the second boundary condition, following the phenomenological derivation of the Cahn–Hilliard system, we consider, in addition to the usual Ginzburg–Landau free energy and assuming that the interactions with the walls are short-ranged, a surface free energy of the form
ΨΓ(u,∇Γu)=∫Γ(αΓ2|∇Γu|2+G(u))dσ, αΓ>0, | (2.76) |
where ∇Γ is the surface gradient and G is a surface potential. Thus, the total free energy of the system reads
Ψ=ΨΩ+ΨΓ. | (2.77) |
Writing finally that the system tends to minimize the excess surface energy, we are led to postulate the following boundary condition:
1d∂u∂t−αΓΔΓu+g(u)+α∂u∂ν=0, on Γ, | (2.78) |
i.e., there is a relaxation dynamics on the boundary (note that it follows from the boundary conditions that
dΨdt=−1κ‖∂u∂t‖2H−1(Ω)−1d‖∂u∂t‖2L2(Γ)≤0), |
where ΔΓ is the Laplace–Beltrami operator, g=G′ and d>0 is some relaxation parameter, which is usually referred to as dynamic boundary condition, in the sense that the kinetics, i.e., ∂u∂t, appears explicitly. Furthermore, in the original derivation, one has G(s)=12aΓs2−bΓs, where aΓ>0 accounts for a modification of the effective interaction between the components at the walls and bΓ characterizes the possible preferential attraction (or repulsion) of one of the components by the walls (when bΓ vanishes, there is no preferential attraction). We also refer the reader to [26,157] for other physical derivations of the dynamic boundary condition, obtained by taking the continuum limit of lattice models within a direct mean-field approximation and by applying a density functional theory, respectively, to [328] for the derivation of dynamic boundary conditions in the context of two-phase fluid flows and to [337,341] for an approach based on concentrated capacity.
Remark 2.14. Actually, it would seem more reasonable, in the case of nonpermeable walls, to write the conservation of mass both in the bulk Ω and on the boundary Γ, i.e.,
ddt(∫Ωudx+∫Γudσ)=0. |
Indeed, due to the interactions with the walls, one should expect some mass on the boundary. We assume that the first equation of (1.1) still holds. Then, writing that
μ=∂uΨ, |
where ∂ is the variational derivative mentioned above (note that, in the original derivation, one has μ=∂uΨΩ), we obtain the second equation of (1.1), together with the boundary condition
μ=−αΓΔΓu+g(u)+α∂u∂ν, on Γ. |
We now note that, owing to the first equation of (1.1), the above mass conservation reads
∫Γ(∂u∂t+κ∂μ∂ν)dσ=0. |
A class of boundary conditions which ensure this mass conservation reads
∂u∂t+βΓΔΓu+κ∂μ∂ν=0, on Γ, βΓ≥0. |
We can thus see that, when βΓ>0, we also have a Cahn–Hilliard type system on the boundary. Note that, when βΓ=0, it follows from the above that
dΨdt=−κ‖∇μ‖2L2(Ω)n≤0. |
We refer the reader to [77,197] for the study of this problem (see also [282,291] for higher-order models and [163,164,172] for similar dynamic boundary conditions in the case of semipermeable walls).
Again, for regular nonlinear terms, the problem is well understood from a mathematical point of view (see, e.g., [88,163,164,172,302,326,329,368]).
The first proof of existence of solutions to the Cahn–Hilliard equation with singular (and, in particular, logarithmic) potentials and dynamic boundary conditions is given in n [190] (see also [191]), assuming that the (regular in our case; see [104,190] for singular surface nonlinear terms) surface nonlinearity g has the right sign at the singular points of the bulk nonlinearity f, namely,
±g(±1)>0 | (2.79) |
(see also [80] for a similar result for the Caginalp phase-field system; note that the Cahn–Hilliard equation can also be derived as a singular limit of the Caginalp phase-field system, see [54,55,56]). Roughly speaking, these conditions force the order parameter to stay away from the pure states ±1 on the boundary.
A first natural question is what happens when the above sign conditions are not satisfied.
An important feature of the Cahn–Hilliard equation with a singular potential and dynamic boundary conditions is that one can have nonexistence of classical (i.e., in the sense of distributions) solutions (of course, when the sign conditions (2.79) are not satisfied), already in one space dimension.
We will illustrate this by considering the following simple scalar ODE:
y″−f(y)=0, in (−1,1), y′(±1)=K>0. | (2.80) |
We assume that f is odd and singular at ±1 and that F has finite limits at ±1 (here, F is any antiderivative of f). In particular, these assumptions are satisfied by the physically relevant logarithmic potentials.
Then, when K is small, one has the existence and uniqueness of a (classical) solution to (2.80) which is separated from the singular values of f (i.e., ‖y‖L∞(−1,1)<1). Furthermore, it follows from standard interior regularity estimates that
|y′(x)|≤c0, x∈(−12,12), | (2.81) |
where the positive constant c0 is independent of K.
Multiplying (2.80) by y′ and integrating over (0,1), we obtain
|12K2−F(y(1))|≤c1, | (2.82) |
where, owing to (2.81), the positive constant c1 is independent of K. Since F is bounded, independently of K, this shows that the above inequality cannot hold when K is large, meaning that there cannot be a classical solution to (2.80).
Finally, noting that y is odd, we can rewrite (2.80) in the equivalent form
y″−f(y)=⟨y″−f(y)⟩, in (−1,1), y′(±1)=K, |
which corresponds to the one-dimensional stationary Cahn–Hilliard equation (with κ=α=1) with dynamic boundary conditions (with surface potential g≡−K; note that, in one space dimension, the Laplace–Beltrami operator does not make sense and does not appear).
Thus, when the sign conditions are not satisfied, we should expect to have nonexistence of classical solutions. However, we will see below that, approximating the singular nonlinear term by regular ones, we can prove that, at least for a subsequence, the corresponding solutions converge to some limit function.
We first rewrite the problem in the following form (where, for simplicity, we have set all physical constants equal to 1):
{∂u∂t=Δμ, ∂μ∂ν|Γ=0,μ=−Δu+f0(u)+λu, λ∈R,∂v∂t−ΔΓv+g0(v)+v+∂u∂ν=0, on Γ, v=u|Γ, | (2.83) |
where f=f0+λI and g=g0+I.
We then make the following assumptions:
f0∈C2(−1,1), f0(0)=0, f′0≥0, sgn(s)f″0(s)≥0, s∈(−1,1), | (2.84) |
lims→±1f0(s)=±∞, lims→±1f′0(s)=+∞, | (2.85) |
g0∈C2(R), ‖g0‖C2(R)<+∞. | (2.86) |
We can note that the physically relevant logarithmic functions f (1.4) can indeed be decomposed into a sum f0+λI, where f0 satisfies the above assumptions.
We now introduce, as above, the following regular approximations of f0, for N∈N:
f0,N(s)={f0(s), |s|≤1−1N,f0(1−1N)+f′0(1−1N)(s−1+1N), s>1−1N,f0(−1+1N)+f′0(−1+1N)(s+1−1N), s<−1+1N, | (2.87) |
and we consider (2.83) in which f0 is replaced by f0,N, N∈N.
The existence, uniqueness and regularity of the solution uN to this regularized problem is clear, since the nonlinear term is now regular (see [302]). Furthermore, we have the following estimates, for N large enough:
‖uN(t)‖2Cη(Ω)+‖uN(t)‖2H2(Γ)+‖uN(t)‖2H2(Ωε)+‖uN(t)‖2H1(Ω)+‖∂uN∂t(t)‖2H−1(Ω) | (2.88) |
+‖∂uN∂t(t)‖2L2(Γ)+‖∇DτuN(t)‖2L2(Ω)(n−1)n+‖f0,N(uN(t))‖L1(Ω) |
∫t+1t(‖∂uN∂t(s)‖2H1(Ω)+‖∂uN∂t(s)‖2H1(Γ))ds |
≤c1e−c2t(1+‖uN(0)‖2H1(Ω)+‖uN(0)‖2H1(Γ)+‖∂uN∂t(0)‖2H−1(Ω)+‖∂uN∂t(0)‖2L2(Γ))2+c3, |
where Ωε={x∈Ω, dist(x,Γ)>ε}, ε>0, DτuN=∇uN−∂uN∂νν is the tangential part of the gradient (here, ν also denotes a smooth extension of the unit outer normal to the boundary in Ω) and the positive constants η<14 and ci, i=1,\..., 3, are independent of N.
The only difficulty, to derive these estimates, is to obtain the estimate on the tangential part of the gradient and the interior H2-estimate. This is achieved by a proper variant of the nonlinear localization technique, see [305] for details.
Remark 2.15. Actually, uN also belongs to H2(Ω), but the H2-norm of uN depends a priori on N and such a regularity does not pass to the limit.
We also have the following (parabolic) regularization property on the solution uN to the regularized problem:
‖∂uN∂t(t)‖2H−1(Ω)+‖∂uN∂t(t)‖2L2(Γ) | (2.89) |
≤ct(1+‖uN(0)−⟨uN(0)⟩‖2H−1(Ω)+‖uN(0)‖2L2(Γ)), t∈(0,1], |
where the positive constant c is independent of N.
Finally, for any two solutions u1 and u2 to the regularized problem (for simplicity, we omit the index N here), with initial data having the same average (note that we still have the conservation of the average when considering dynamic boundary conditions), there holds
‖u1(t)−u2(t)‖H−1(Ω)+‖u1(t)−u2(t)‖L2(Γ) | (2.90) |
≤cec′t(‖u1(0)−u2(0)‖H−1(Ω)+‖u1(0)−u2(0)‖L2(Γ)), ∀t≥0, |
where the positive constants c and c′ are independent of t, N and u1 and u2.
In particular, it follows from (2.88) that, at least for a subsequence which we do not relabel, uN converges (at least weakly) to some function u in the corresponding spaces. Now, recalling that one expects nonexistence of classical solutions in general, u cannot be a (classical) solution to the Cahn–Hilliard system (2.83) with the original singular nonlinearity f0 in general. However, we will see below that uN converges to the solution to some variational inequality, derived from (2.83).
Our aim now is to pass rigorously to the limit in the regularized problems associated with (2.83). As already mentioned, as the limit is not a classical solution to (2.83) in general, we first need to define a proper weak formulation of the problem. More precisely, this will be done by considering a variational inequality (see also [197,209] for a very close approach, but at an abstract level, i.e., based on duality arguments).
To do so, we first introduce the bilinear form
B(w,z)=((∇w,∇z))Ω+λ((w,z))Ω+L(((−Δ)−1¯w,¯z))Ω+((∇Γw,∇Γz))Γ, |
(w,z)∈H1(Ω)⊗H1(Γ)={q∈H1(Ω), q|Γ∈H1(Γ)}, where the positive constant L is chosen such that the following coercivity relation holds:
‖∇w‖2L2(Ω)n+λ‖w‖2L2(Ω)+L‖w‖2H−1(Ω)≥12‖w‖2H1(Ω), ∀w∈H1(Ω) such that ⟨w⟩=0. |
Furthermore, −Δ denotes again the minus Laplace operator with Neumann boundary conditions and acting on functions with null average, ¯w=w−⟨w⟩ and ((⋅,⋅))Ω and ((⋅,⋅))Γ denote the scalar products in L2(Ω) and L2(Γ), respectively.
We then rewrite the problem in the following equivalent form:
{(−Δ)−1∂u∂t−Δu+f0(u)+λu−⟨μ⟩=0,μ=−Δu+f0(u)+λu,∂v∂t−ΔΓv+g(v)+∂u∂ν=0, on Γ, v=u|Γ,u|t=0=u0, v|t=0=v0. | (2.91) |
We multiply the first equation of (2.91) by u−w, where w=w(x) is such that
⟨u(t)−w⟩=0, ∀t≥0, |
and have, owing to the boundary conditions,
(((−Δ)−1∂u∂t,u−w))Ω+((∂u∂t,u−w))Γ+B(u,u−w)+((f0(u),u−w))Ω |
=L((u,(−Δ)−1(u−w)))Ω−((g(u),u−w))Γ. |
Noting that B is positive and f0 is monotone increasing, we finally obtain the following variational inequality:
(((−Δ)−1∂u∂t,u−w))Ω+((∂u∂t,u−w))Γ+B(w,u−w)+((f0(w),u−w))Ω | (2.92) |
≤L((u,(−Δ)−1(u−w)))Ω−((g(u),u−w))Γ |
(what is important here, when considering a singular nonlinear term f0, is that this function acts on the test functions).
We now introduce the phase space
Φ={(q,r)∈L∞(Ω)×L∞(Γ), ‖q‖L∞(Ω)≤1, ‖r‖L∞(Γ)≤1} |
and are in a position to give the definition of a variational (weak) solution.
Definition 2.16. Let (u0,v0) belong to Φ. Then, a pair (u,v) is a variational solution to (2.91) if
(ⅰ) (u,v)∈C([0,+∞);H−1(Ω)×L2(Γ))∩L2(0,T;H1(Ω)×H1(Γ)), ∀T>0.
(ⅱ) (∂u∂t,∂v∂t)∈L2(τ,T;H−1(Ω)×L2(Γ)), ∀0<τ<T.
(ⅲ) f(u)∈L1((0,T)×Ω), ∀T>0.
(ⅳ) −1<u(t,x)<1, for almost every (t,x)∈R+×Ω.
(ⅴ) u(0)=u0, v(0)=v0.
(ⅵ) ⟨u(t)⟩=⟨u0⟩, ∀t≥0.
(ⅶ) u(t)|Γ=v(t), for almost every t>0.
(ⅷ) The variational inequality (2.92) is satisfied for almost every t>0 and for every test function w=w(x) such that w∈H1(Ω)⊗H1(Γ), f(w)∈L1(Ω) and ⟨w⟩=⟨u0⟩.
Remark 2.17. Of course, a classical solution is a variational one. Furthermore, the notion of a variational solution also makes sense when f0 is regular and, in that case, the two notions of solutions are equivalent (see also [130]).
Remark 2.18. We can note that, in the above definition, u(t)|Γ=v(t) only for t>0 and this condition does not necessarily hold for the initial data. However, as soon as t>0, v can be found, once u is known. This also justifies that we wrote the variational inequality (2.92) in terms of u only.
We can now write the variational inequality (2.92) with u replaced by (a proper subsequence of) the solutions uN to the regularized problems (when u0 is not strictly separated from ±1 or u0|Γ≠v0, we approximate the initial data by a sequence of smooth functions which satisfy these conditions) and, passing to the limit (owing to (2.88); one can proceed as in the proof of Theorem 2.6 to prove the separation property here), we have the
Theorem 2.19. For every pair of initial data (u0,v0)∈Φ, (2.91) possesses a unique variational solution (u,v) which is the limit of a sequence of solutions to the regularized problems and which satisfies (2.88), the regularization property (2.89) and the Lipschitz continuity property (2.90).
This result allows to define a semigroup S(t) acting on the phase space Φ and associated with the variational solutions to (2.91). Furthermore, this semigroup is Lipschitz continuous in the following sense:
‖S(t)(u1,v1)−S(t)(u2,v2)‖H−1(Ω)×L2(Γ)≤cec′t‖(u1,v1)−(u2,v2)‖H−1(Ω)×L2(Γ), t≥0, | (2.93) |
∀(u1,v1), (u2,v2)∈Φ such that ⟨u1⟩=⟨u2⟩.
Remark 2.20. We refer the reader to [305] for the study of finite-dimensional attractors for the semigroup S(t).
Now, as already mentioned several times, a variational solution does not necessarily solve the Cahn–Hilliard system in the usual sense (this would be true if we had an H2-regularity on u, but, here, we a priori only have an interior H2-regularity, together with an L2-estimate on the gradient of the tangential derivatives). Actually, we can be more precise. Indeed, we can prove that a variational solution solves the bulk equation, namely,
(−Δ)−1∂u∂t−Δu+f0(u)+λu−⟨μ⟩=0, |
in the sense of distributions (and almost everywhere). However, it does not necessarily satisfy the dynamic boundary condition.
Again, we can be more precise. First, it follows from (2.88) (for u) that the trace
[∂u∂ν]int=∂u∂ν |
exists, say, in L∞(τ,T;L1(Γ)), 0<τ<T. Furthermore, the (proper subsequence of the) solutions to the regularized problems satisfy the dynamic boundary condition
∂vN∂t−ΔΓvN+g(vN)+∂uN∂ν=0, on Γ, vN=uN|Γ, |
in L∞(τ,T;L2(Γ)), 0<τ<T. We can then pass to the limit in this equation, which yields that the limit
[∂u∂ν]ext=limk→+∞∂uN∂ν |
exists in L∞(τ,T;L2(Ω)) weak star, 0<τ<T, whence, at the limit
∂v∂t−ΔΓv+g(v)+[∂u∂ν]ext=0, on Γ, |
almost everywhere, where [∂u∂ν]ext and [∂u∂ν]int do not necessarily coincide; in particular, a variational solution is a classical one when these two quantities coincide almost everywhere on the boundary.
Remark 2.21. Coming back to the scalar ODE considered in the beginning of this subsection, namely,
y″−f(y)=0, in (−1,1), y′(±1)=K>0, |
we can prove that there exists a critical value K0 of K such that, if K>K0, there is no classical solution. However, there exists a variational solution which is solution to the ODE
y″−f(y)=0, in (−1,1), y(±1)=±1, |
and, in that case,
y′|x=±1≠K. |
It is now natural and important to find sufficient conditions which ensure that a variational solution is a classical one (one such sufficient condition being the sign conditions (2.79) mentioned above). We saw that this is the case when the two quantities [∂u∂ν]ext and [∂u∂ν]int coincide almost everywhere on Γ. In particular, this is the case when u(t) belongs to H2(Ω), for almost every t>0, which, in turn, is related to the (strict) separation from the singularities. Indeed, we have the following result.
Theorem 2.22. Let (u,v) be a variational solution and set, for δ∈(0,1) and T>0,
Ωδ(T)={x∈Ω, |u(T,x)|<1−δ}. |
Then, u(T)∈H2(Ωδ(T)) and
‖u(T)‖H2(Ωδ(T))≤cδ,T, |
where cδ,T is independent of u.
In particular, it follows from Theorem 2.22 that u(t) is H2-regular in each subdomain in which it is strictly separated from ±1. Furthermore, a consequence of this result is that, if
|u(t,x)|<1, for almost every (t,x)∈R+×Γ, | (2.94) |
then
[∂u∂ν]ext=[∂u∂ν]int, for almost every (t,x)∈R+×Γ, |
and a variational solution is a classical one. We thus finally see that the existence of a classical solution is related to the separation of u from the singularities of the nonlinear term, now on the boundary Γ.
Such a separation holds when f0 has sufficiently strong singularities (see also [78] for a similar result for the Caginalp phase-field system). More precisely, we have the
Theorem 2.23. We assume that
lims→±1F0(s)=+∞, |
where F0 is any antiderivative of f0. Then, (2.94) holds and a variational solution is a classical one.
In particular, this holds when f0 has a growth of the form
±1(1−s2)p, p>1, |
close to the singular points ±1. Unfortunately, for the relevant logarithmic potentials, F0 is bounded, so that this theorem cannot be applied. In that case, we can have |u(t,x)|=1 on a set with nonzero measure on the boundary, or even on the whole boundary (see also the scalar ODE considered above).
We finally recall the
Theorem 2.24. We assume that
±g(±1)>0. |
Then, a variational solution is a classical one.
As already mentioned, the sign conditions force the order parameter to stay away from the pure states on the boundary.
We mention in this subsection several important generalizations of the Cahn–Hilliard equation.
A first one consists in studying systems of Cahn–Hilliard equations to describe phase separation in multicomponent alloys (see [51,91,107,139,140,146,178,179,180,298]).
We also mention the stochastic Cahn–Hilliard equation (also called the Cahn–Hilliard–Cook equation) which takes into account thermal fluctuations (see [29,30,32,33,63,110,112,117,118,133,202,203,219]).
Then, an important generalization of the Cahn–Hilliard equation is the viscous Cahn–Hilliard equation which accounts for viscosity effects in the phase separation of polymer/polymer systems (see [16,65,93,142,310]). The viscous Cahn–Hilliard equation can also be seen as a particular case of the generalizations proposed by M. Gurtin in [221] (which, in particular, account for anisotropy) and which are based on a microforce balance, i.e., a new balance law for interactions at a microscopic level (see [36,37,39,79,130,131,196,206,284,285,286,294,295,299,304,332,333,334,364] for the mathematical analysis); we also refer the reader to yet another approach proposed by P. Podio–Guidugli in [325] and studied in, e.g., [97,98,99,100,105].
Another important generalization of the Cahn–Hilliard equation is the hyperbolic relaxation of the equation, proposed in [174,175,176,177,260] to model the early stages of spinodal decomposition in certain glasses (see also [38,184,185,210,211,212,340] for the mathematical analysis and [338,339] for the hyperbolic relaxation of the Cahn–Hilliard–Oono equation in the whole space). Actually, the hyperbolic relaxation of the equation is a particular case of more general memory relaxations (for an exponentially decreasing memory kernel) which were studied, e.g., in [106,109,186,187] (see also [327]).
We also mention the convective Cahn–Hilliard equation which describes the dynamics of driven systems such as faceting of growing thermodynamically unstable crystal surfaces (see [126,127,128,198,267,361] for the mathematical analysis).
It is important to note that, in realistic physical systems, quenches are usually carried out over a finite period of time, so that phase separation can begin before the final quenching is reached. It is thus important to consider nonisothermal Cahn–Hilliard models. Such models were derived and studied in [8,9,170,171,297,346].
The Cahn–Hilliard equation can be coupled with the Allen–Cahn equation which describes the ordering of atoms during the phase separation process (see [7]). This problem was studied, e.g., in [28,114,269,296,312,374].
It can also be coupled with the equations for elasticity or viscoelasticity, to account for mechanical effects (see, e.g., [12,27,34,35,64,121,179,180,181,284,285,318,319,320,321,331]).
We also mention the coupling of the Cahn–Hilliard equation with the Navier–Stokes equations in the context of two-phase (multiphase) flows (see, e.g., [1,3,43,44,45,46,47,49,61,62,86,94,158,166,167,169,195,222,236,247,250,252,268,273,372,375]) and some related models such as the Cahn–Hilliard– Hele–Shaw and Cahn–Hilliard–Brinkman equations (see, e.g., [42,108,119,120,153,193,225,359,360,365,371]). Related models can also be used to model tumor growth (see, e.g., [96,101,102,103,113,159,182,237,272]).
We finally refer the reader to, e.g., [5,6,10,11,16,17,18,19,20,21,22,40,46,47,48,49,50,52,67,69,71,87,89,111,122,135,136,137,141,147,150,151,152,154, 159,161,183,199,204,205,207,220,223,224,226,230,231,242,243,246,247,248,249,250,251,252,261,262,263,265,266, 270,275,280,283,306,330,336,344,345,347,351,358,362,366,369,377,378] for the numerical analysis and simulations of the Cahn–Hilliard equation (and several of its generalizations).
We consider the following initial and boundary value problem in a bounded and regular domain Ω of Rn, n=1, 2 or 3, with boundary Γ:
∂u∂t+Δ2u−Δf(u)+g(u)=0, | (3.1) |
∂u∂ν=∂Δu∂ν=0, on Γ, | (3.2) |
u|t=0=u0, | (3.3) |
where f is a smooth function defined on R (as already mentioned, typically, f(s)=s3−s) and
g(s)=∑qi=0bisi, bq≠0, q≥2. | (3.4) |
The main feature of (3.1)-(3.2), together with a function g as in (3.4), is that we can have blow up in finite time.
In order to exhibit blow up in finite time, we look for spatially homogeneous solutions, i.e., solutions of the form
u(t,x)=y(t), |
whence the ODE
y′+∑qi=0biyi=0. | (3.5) |
Let x0<x1<⋅⋅⋅<xk be the real roots of g (we assume in what follows that k≥1, though the case k=0 is also contained in Theorem 3.1 below; see also Remark 3.2). We thus have
g(s)=bq∏ki=1(s−xi)αi∏ri=1(s2+λis+βi)ui | (3.6) |
and
1g(s)=1bq[∑ki=1(∑αij=1αi,j(s−xi)j)+∑ri=1(∑uij=1bi,js+ci,j(s2+λis+βi)j)] | (3.7) |
(here, we assume, without loss of generality, that r≥1).
Therefore, (3.5) is equivalent to
ψ(y)=bq(−t+κ), | (3.8) |
where ψ is an antiderivative of bqg(s) and
κ=1bqψ(y0), y0=y(0). | (3.9) |
Let ˜k be the number of roots of g which have an odd order (i.e., for which αi is odd).
We have the
Theorem 3.1. We assume that ˜k is even. Then, we have blow up in finite time.
Proof. We first note that ψ has finite limits λ± as s tends to ±∞. Indeed, the only terms in (3.7) which yield infinite limits when taking an antiderivative can be written as
∑ki=1αi,1s−xi+∑ri=1bi,1s+ci,1s2+λis+βi. |
Then, when taking an antiderivative, we need to deal with the function
h(s)=∑ki=1αi,1ln|s−xi|+∑ri=1bi,12ln(s2+λis+βi). |
Now, noting that it follows from (3.7) that, necessarily,
∑ki=1αi,1+∑ri=1bi,1=0 | (3.10) |
and writing
h(s)=ln(∏ki=1|s−xi|αi,1∏ri=1(s2+λis+βi)bi,12), |
it follows from (3.10) that
lims→±∞h(s)=0. | (3.11) |
Furthermore, since ˜k is even, then ψ is monotone increasing on ]−∞,x1[ and ψ(]−∞,x1[)=]λ−,+∞[. Similarly, ψ is monotone increasing on ]xk,+∞[ and ψ(]xk,+∞[)=]−∞,λ+[.
Let us first assume that bq>0. In that case, we take y0<x1 and there is a local (in time) solution to (3.5), with initial datum y0 (as long as y(t)<x1). Moreover,
y(t)=ψ−1(bq(−t+κ)) | (3.12) |
and this solution exists as long as
bq(−t+κ)>λ−, |
i.e.,
t<κ−λ−bq, | (3.13) |
meaning that we have blow up in finite time.
Similarly, if bq<0, we take y0>xk and we have a solution as long as
bq(−t+κ)<λ+, |
i.e.,
t<κ−λ+bq, | (3.14) |
whence again blow up in finite time.
Remark 3.2. If k=0, then ψ maps increasingly R onto ]λ−,λ+[ and we can easily conclude, proceeding as above and taking y0 arbitrarily.
Now, when ˜k is odd, we have the
Theorem 3.3. We assume that ˜k is odd and bq<0. Then, we have blow up in finite time.
Proof. Proceeding as above, we see that ψ is monotone decreasing on ]−∞,x1[ and ψ(]−∞,x1[)=]−∞,λ−[. Taking y0<x1, we have a solution to (3.5) as long as
bq(−t+κ)<λ−, |
i.e.,
t<κ−λ−bq, | (3.15) |
meaning once more that we have blow up in finite time.
Remark 3.4. More generally, we have blow up in finite time whenever g is continuous on an interval ]−∞,x0[ (resp., ]x0,+∞[) and maps increasingly (resp., decreasingly) ]−∞,x0[ (resp, ]x0,+∞[) onto ]λ,+∞[. Here, λ is finite.
Example 3.5. We take
g(s)=λs(s−1), λ>0. | (3.16) |
In that case, (3.1) has applications in wound healing and tumor growth and λ is a proliferation coefficient (see [244]). Here, ˜k=k=2 and bq=λ>0. It thus follows from Theorem 3.1 that we can have blow up in finite time (see also [85]). Furthermore, here, x0=0, so that blow up in finite time occurs when y0<0. We can note that, in this example, the biologically relevant interval is [0,1], so that a natural question is whether we can have blow up in finite time in (3.1) for initial data u0 such that u0(x)∈[0,1], a.e. in Ω. Numerical simulations performed in [85] suggest that this can indeed happen. Actually, what is important here is the choice of the nonlinear term f and, more precisely, the minima of the double-well potential F (we recall that f=F′).
Example 3.6. We take
g(s)=λd2(1+s)−λg(1+s)2(1−s)2, λd, λg>0. | (3.17) |
In that case, (3.1) has biological applications and λd and λg are death and growth coefficients, respectively (see [14]). Furthermore, a study of the function g shows that either ˜k=k=4 or ˜k=2 and k=2 or 3. Noting that bq=−λg<0, it follows from Theorem 3.1 that we can have blow up in finite time which occurs when y0>1 (indeed, it is easy to show that, in this example, xk>1). Here, the biologically relevant interval is [−1,1] and, again, a natural question is whether we can have blow up in finite time for (3.1) when u0(x)∈[−1,1], a.e. in Ω. Numerical simulations suggest that, in that case, the solutions remain in the biologically relevant interval (see [14,149]).
Remark 3.7. Another interesting question is whether the solutions to (3.1) remain in the biologically relevant interval, assuming that the initial condition u0 also belongs to this interval. It was proved in [85] that, for (3.16), this may not be the case (see also [324] for the Cahn–Hilliard equation). Let us now consider the function g defined in (3.17) and assume that f(s)=s3−s. In one space dimension, (3.1) then reads, with obvious notation,
ut+uxxxx−(u3−u)xx+g(u)=0. | (3.18) |
We take the initial datum u0 such that u0(x)=1−1+λd24x4 in a neighborhood of 0 and extend it to a smooth function defined on (−1,1) and taking values in [−1,1]. We note that u0,x(0)=u0,xx(0)=0, while u0,xxxx=−1−λd. It thus follows from (3.18) that ut(0,0)=1, so that
u0,t=1+t+o(t). |
Therefore, u(0,t)>1 for t>0 small, meaning that u does not stay in the biologically relevant interval.
Remark 3.8. The above results also show that we can have blow up in finite time for the reaction-diffusion equation
∂u∂t−Δu+g(u)=0, | (3.19) |
associated with the Neumann boundary condition ∂u∂ν=0, on Γ, which is also relevant in view of biological applications. Actually, we can say more here. Indeed, let u0∈L∞(Ω) be an initial datum for (3.19) and let y± be the solutions to the ODE's
y′±+g(y±)=0, y±(0)=y±,0, | (3.20) |
where y−,0≤u0(x)≤y+,0, a.e. in Ω. Then, it follows from the comparison principle for second-order parabolic equations that
y−(t)≤u(t,x)≤y+(t), | (3.21) |
meaning that, if u0 is properly chosen, u blows up in finite time. Similarly, the comparison principle also shows that, when u0 is properly chosen (i.e., when y±,0 yield solutions to (3.5) which do not blow up in finite time), then we have global (in time) existence; in particular, in the two examples above, we have global (in time) existence when u0 remains in the biologically relevant interval. Now, such a comparison principle does not hold for fourth-order parabolic equations, so that the results obtained in Theorems 3.1 and 3.3 do not say more on the qualitative behavior of the solutions to (3.1) in general. However, in [85], we were able to obtain a more complete picture in the particular case (3.16) by studying the evolution equation for the spatial average of u. More precisely, we proved that, if u is a solution to (3.1)-(3.2), then either u blows up in finite time or u exists globally in time and 0≤⟨u(t)⟩≤⟨u0⟩+1, ∀t≥0. Furthermore, if u is a nonvanishing solution to (3.1)-(3.2) such that u(t)∈[0,1], ∀t≥0, then u tends to 1 in H1(Ω) as t→+∞. For a more general source term g (even polynomial), this seems much more complicated and will be studied elsewhere (see also [148,149]).
Remark 3.9. When ˜k is odd and bq>0, then we do not have blow up in finite time. Indeed, in that case, necessarily, q is odd, q≥3, so that (3.5) is dissipative. Indeed, multiplying (3.5) by y, we easily obtain
ddty2+bqyq+1≤c, | (3.22) |
whence, in particular,
ddty2+cy2≤c′, c>0. | (3.23) |
Here and below, the same letters c and c′ (and also c″) denote constants which may change from line to line. We thus deduce from (3.23) that
y2(t)≤y20e−ct+c′, c>0, | (3.24) |
and the solutions to (3.5) are indeed global in time. Furthermore, multiplying (3.1) by u and integrating over Ω, we find, assuming that the standard dissipativity assumption
f′≥−c0, c0≥0, | (3.25) |
holds, a differential inequality of the form
ddt‖u‖2L2(Ω)+‖Δu‖2L2(Ω)+bq‖u‖q+1Lq+1(Ω)≤2c0‖∇u‖2L2(Ω)n+c. | (3.26) |
It follows from (3.26) that
ddt‖u‖2L2(Ω)+c‖u‖2H2(Ω)+bq2‖u‖q+1Lq+1(Ω)≤c′‖u‖2H1(Ω)+c″, c>0. | (3.27) |
Employing the interpolation inequality
‖u‖H1(Ω)≤c‖u‖12L2(Ω)‖u‖12H2(Ω), |
we deduce that
ddt‖u‖2L2(Ω)+c‖u‖2H2(Ω)+bq2‖u‖q+1Lq+1(Ω)≤c′‖u‖2L2(Ω)+c″, |
whence, owing to Young's inequality,
ddt‖u‖2L2(Ω)+c‖u‖2H2(Ω)+bq4‖u‖q+1Lq+1(Ω)≤c′, c>0. | (3.28) |
This yields that a solution to (3.1)-(3.2) (when it exists) is global in time and is dissipative in L2(Ω) (in the sense that it follows from Gronwall's lemma that ‖u(t)‖2L2(Ω) is bounded independently of time and bounded sets of initial data for t large).
We consider in this section the following generalization of the Cahn–Hilliard equation introduced in [24] in view of applications in image inpainting:
∂u∂t+Δ2u−Δf(u)+χΩ∖D(x)(u−h)=0, | (4.1) |
where f is, for simplicity, the cubic function f(s)=s3−s and h∈L2(Ω) (actually, we will take no image, h≡0, for simplicity). Here, we have taken all parameters equal to 1. This equation is endowed with the usual Neumann boundary conditions and the initial condition u|t=0=u0. Furthermore, D is an open bounded subset of Ω such that D⊂⊂Ω and χ denotes the indicator function.
The first existence and uniqueness result was obtained in [25]. Then, to go further and, in particular, to prove the existence of finite-dimensional attractors, we need to derive a global in time and dissipative estimate. Obtaining such an estimate is not straightforward, due to the fact that we no longer have the conservation of mass.
Indeed, integrating (4.1) over Ω, we have
d⟨u⟩dt+1Vol(Ω)∫Ω∖Dudx=0. |
In order to deal with this equation, we write
u=⟨u⟩+v, |
where v satisfies the equation
∂∂t(−Δ)−1v−Δv+f(⟨u⟩+v)−⟨f(⟨u⟩+v)⟩ |
+(−Δ)−1(χΩ∖D(x)u−⟨χΩ∖D(x)u⟩)=0. |
Furthermore, we can see that
d⟨u⟩dt+c0⟨u⟩=−1Vol(Ω)∫Ω∖Dvdx, c0=Vol(Ω∖D)Vol(Ω). |
The left-hand side of the above equation is the simplest dissipative ODE and there just remains to control the right-hand side in order to have a global in time and dissipative estimate. To do so, we multiply the equation for v by v and integrate over Ω and by parts. However, in order to absorb bad terms which appear, we need some coercivity on the nonlinear term. More precisely, we write that
((f(⟨u⟩+v)−⟨f(⟨u⟩+v)⟩,v))=((f(⟨u⟩+v)−f(⟨u⟩),v)) |
≥c02∫Ω(v4+v2⟨u⟩2)dx−‖v‖2, |
where ((⋅,⋅)) again denotes the usual L2-scalar product, with associated norm ‖⋅‖. This then allows to have a global in time and dissipative estimate on v, then on ⟨u⟩ and finally on u. Having this, we can go further and obtain further regularity results and the existence of finite-dimensional attractors. We refer the reader to [73] for more details.
Remark 4.1. The question of the convergence of single trajectories to steady states is an important open problem. This question is all the more important that the final inpainting result is expected to be a steady state of the equation.
Now, again, the case of the thermodynamically relevant logarithmic nonlinear terms is much more involved. Considering such nonlinear terms is relevant here. Indeed, numerical simulations performed in [74] suggest better inpainting results as far as the convergence time is concerned. Furthermore, the final inpainting result is much better, when the inpainting domain D is large.
In what follows, we again take h≡0. However, for a nonvanishing image h, we would need a condition of the form
∫Ω∖Dhdx=0, |
meaning that we need some kind of symmetry.
We have the
Theorem 4.2. We assume that u0∈H1(Ω), |⟨u0⟩|<1 and −1<u0(x)<1, a.e. x∈Ω. Then, there exists T0=T0(u0) and a solution to the problem on [0,T0] such that u∈C([0,T0];H−1(Ω))∩L∞(0,T0;H1(Ω))∩L2(0,T0;H2(Ω)) and ∂u∂t∈L2(0,T0;H−1(Ω)). Furthermore, −1<u(t,x)<1, a.e. (t,x)∈(0,T0)×Ω.
Proof. The proof is similar to the one performed in Section 2. However, we need to approximate the logarithmic nonlinear term in a careful way, as we need a coercivity property which is similar to the one obtained for the usual cubic nonlinear term for the approximated functions; this coercivity also needs to be uniform with respect to the approximation parameter.
To do so, we write (see (1.3)) F(s)=θc2(1−s2)+F1(s) and f1=F′1. We then introduce, following [158] and for N∈N, the approximated functions F1,N∈C4(R) defined by
F(4)1,N(s)={F(4)1(1−1N), s>1−1N,F(4)1(s), |s|≤1−1N,F(4)1(−1+1N), s<−1+1N, | (4.2) |
F(k)1,N(0)=F(k)1(0), k=0, 1, 2, 3, | (4.3) |
so that
F1,N(s)={∑4k=01k!F(k)1(1−1N)(s−1+1N)k, s>1−1N,F1(s), |s|≤1−1N,∑4k=01k!F(k)1(−1+1N)(s+1−1N)k, s<−1+1N. | (4.4) |
Setting FN(s)=θc2(1−s2)+F1,N(s), f1,N=F′1,N and fN=F′N, there holds
f′1,N≥0, f′N≥−θc, | (4.5) |
FN≥−c1, c1≥0, | (4.6) |
fN(s)s≥c2(FN(s)+|fN(s)|)−c3, c2>0, c3≥0, s∈R, | (4.7) |
where the constants ci, i=1, 2 and 3, are independent of N, for N large enough. Furthermore, there holds, for N large enough,
(fN(s+a)−fN(a))s≥c4(s4+a2s2)−c5, c4>0, c5≥0, s, a∈R, | (4.8) |
where the constants c4 and c5 are independent of N, which is the required coercivity property (see [74]).
We consider, for N∈N, the approximated problems
∂uN∂t+Δ2uN−ΔfN(uN)+χΩ∖D(x)uN=0, | (4.9) |
∂uN∂ν=∂ΔuN∂ν=0, on Γ, | (4.10) |
uN|t=0=u0. | (4.11) |
We first derive uniform (with respect to N) a priori estimates. In particular, a crucial step is to prove that, at least locally in time, the spatial average of uN is strictly separated from the pure states ±1 and fN(uN) is bounded in L2, which will allow to prove the (local in time) existence of a solution. All constants below are independent of N. Furthermore, the same letters denote constants which may vary from line to line.
First, integrating (4.9) over Ω, we have
d⟨uN⟩dt+1Vol(Ω)∫Ω∖DuNdx=0. | (4.12) |
Setting uN=⟨uN⟩+vN (so that ⟨vN⟩=0), we can rewrite (4.12) as
d⟨uN⟩dt+c0⟨uN⟩=−1Vol(Ω)∫Ω∖DvNdx, | (4.13) |
where, as above, c0=Vol(Ω∖D)Vol(Ω) and vN is solution to
∂vN∂t+Δ2vN−Δ(fN(uN)−⟨fN(uN)⟩)+χΩ∖D(x)uN−⟨χΩ∖D(x)uN⟩=0, | (4.14) |
∂vN∂ν=∂ΔvN∂ν=0, on Γ, | (4.15) |
vN|t=0=v0=u0−⟨u0⟩. | (4.16) |
We rewrite (4.14)-(4.15) in the equivalent form
(−Δ)−1∂vN∂t−ΔvN+fN(uN)−⟨fN(uN)⟩ | (4.17) |
+(−Δ)−1(χΩ∖D(x)uN−⟨χΩ∖D(x)uN⟩)=0, |
∂vN∂ν=0, on Γ. | (4.18) |
We multiply (4.17) by vN to obtain
12ddt‖vN‖2−1+‖∇vN‖2 | (4.19) |
+((fN(uN)−⟨fN(uN)⟩,vN))+((χΩ∖D(x)uN,(−Δ)−1vN))=0. |
Noting that
((fN(uN)−⟨fN(uN)⟩,vN))=((fN(uN)−fN(⟨uN⟩),vN)), |
it follows from (4.8) that
((fN(uN)−⟨fN(uN)⟩,vN))≥c4(‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2)−c. | (4.20) |
Furthermore,
|((χΩ∖D(x)uN,(−Δ)−1vN))|≤c(‖vN‖2+|⟨uN⟩|‖vN‖) | (4.21) |
≤c42(‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2)+c. |
We thus deduce from (4.19)-(4.21) that
ddt‖vN‖2−1+‖∇vN‖2+c4(‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2)≤c. | (4.22) |
Next, it follows from (4.13) that
d⟨uN⟩2dt+c0⟨uN⟩2≤c‖vN‖2, |
whence
d⟨uN⟩2dt+c0⟨uN⟩2≤c42(‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2)+c. | (4.23) |
Summing (4.22) and (4.23), we find a differential inequality of the form
dE1,Ndt+c(‖uN‖2H1(Ω)+‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2)≤c′, c>0, | (4.24) |
where
E1,N=⟨uN⟩2+‖vN‖2−1 |
satisfies
E1,N≥c‖uN‖2H−1(Ω), c>0. | (4.25) |
We then multiply (4.9) by uN and have, owing to (4.5),
ddt‖uN‖2+‖ΔuN‖2≤2θc‖∇uN‖2+c‖uN‖2. | (4.26) |
Summing (4.24) and (4.26) multiplied by δ1, where δ1>0 is chosen small enough, we obtain a differential inequality of the form
dE2,Ndt+c(‖uN‖2H2(Ω)+‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2)≤c′, c>0, | (4.27) |
where
E2,N=δ1‖uN‖2+E1,N |
satisfies
E2,N≥c‖uN‖2, c>0. | (4.28) |
We now rewrite (4.9)-(4.10) in the equivalent form
∂uN∂t+χΩ∖D(x)uN=ΔμN, | (4.29) |
μN=−ΔuN+fN(uN), | (4.30) |
∂uN∂ν=∂μN∂ν=0, on Γ, | (4.31) |
where, by analogy with the original Cahn–Hilliard equation, μN is called chemical potential.
We multiply (4.29) by μN and (4.30) by ∂uN∂t to find
12ddt(‖∇uN‖2+2∫ΩFN(uN)dx)+‖∇μN‖2=−((uN,χΩ∖D(x)μN)). | (4.32) |
Furthermore, multiplying (4.30) by χΩ∖D(x)uN, we have
((uN,χΩ∖D(x)μN))=−((ΔuN,χΩ∖D(x)uN))+∫Ω∖DfN(uN)uNdx. | (4.33) |
We deduce from (4.7) and (4.32)-(4.33) that
ddt(‖∇uN‖2+2∫ΩFN(uN)dx) | (4.34) |
+c(‖∇μN‖2+∫Ω∖D|fN(uN)|dx+∫Ω∖DFN(uN)dx)≤c′‖uN‖2H2(Ω), c>0. |
Summing (4.27) and (4.34) multiplied by δ2, where δ2>0 is chosen small enough, we obtain a differential inequality of the form
dE3,Ndt+c(‖uN‖2H2(Ω)+‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2 | (4.35) |
+∫Ω∖D|fN(uN)|dx+∫Ω∖DFN(uN)dx+‖∇μN‖2)≤c′, c>0, |
where
E3,N=δ2(‖∇uN‖2+2∫ΩFN(uN)dx)+E2,N |
satisfies
E3,N≥c‖uN‖2H1(Ω)−c′, c>0. | (4.36) |
Rewriting (4.29)-(4.30) in the equivalent form
(−Δ)−1∂vN∂t+(−Δ)−1(χΩ∖D(x)uN−⟨χΩ∖D(x)uN⟩)=−(μN−⟨μN⟩), | (4.37) |
μN−⟨μN⟩=−ΔvN+fN(uN)−⟨fN(uN)⟩, | (4.38) |
we deduce from (4.37) that
‖∂vN∂t‖−1≤c(‖uN‖+‖∇μN‖), |
whence, owing to (4.13),
‖∂uN∂t‖H−1(Ω)≤c(‖uN‖+‖∇μN‖). | (4.39) |
Furthermore, (4.38) yields
‖fN(uN)−⟨fN(uN)⟩‖≤c(‖uN‖H2(Ω)+‖∇μN‖). | (4.40) |
It thus follows from (4.35) and (4.39)-(4.40) that
dE3,Ndt+c(‖uN‖2H2(Ω)+‖vN‖4L4(Ω)+⟨uN⟩2‖vN‖2 | (4.41) |
+‖∂uN∂t‖2H−1(Ω)+‖fN(uN)−⟨fN(uN)⟩‖2 |
+∫Ω∖D|fN(uN)|dx+∫Ω∖DFN(uN)dx+‖∇μN‖2)≤c′, c>0. |
We can note that (4.41) is not sufficient to pass to the limit in the nonlinear term fN(uN) (say, in a variational formulation). To do so, we also need an estimate on |⟨fN(uN)⟩| (in order to have an estimate on ‖fN(uN)‖). This could be done if we were able to prove that |⟨uN(t)⟩|≤1−δ, t≥0, δ∈(0,1) (see [301]; see also below). Unfortunately, we are not able to prove such a result and, therefore, we will only be able to obtain a local (in time) result.
We now assume that |⟨u0⟩|<1. Then, there exists δ∈(0,1) such that |⟨u0⟩|≤1−2δ. Therefore, since the function t↦⟨uN(t)⟩ is continuous, there exists T0=T0(δ,N) such that, if t∈[0,T0], then |⟨uN(t)⟩|≤1−δ.
Actually, we can note that it follows from (4.13) that
⟨uN(t)⟩=e−c0t⟨u0⟩−e−c0t∫t0ec0sds∫Ω∖DvNdx, |
so that
|⟨uN(t)⟩|≤|⟨u0⟩|+ce−c0t∫t0ec0s‖uN‖ds | (4.42) |
≤1−2δ+c(1−e−c0t), |
where we emphasize that c=c(u0) is independent of N (note indeed that it follows from (4.27)-(4.28) and Gronwall's lemma that ‖uN‖ is bounded uniformly with respect to time and N). We can thus find T0=T0(δ,u0) independent of N such that, if t∈[0,T0], then |⟨uN(t)⟩|≤1−δ.
Then, noting that we have a similar result for f (see [301]), it is not difficult to prove that, for N large enough,
fN(s+m)s≥c′m|fN(s+m)|−c″m, c′m>0, c″m≥0, s∈R, m∈(−1,1), | (4.43) |
where the constants c′m and c″m depend continuously on m (see also [305]).
Taking s=vN and m=⟨uN⟩ in (4.43), integrating over Ω, noting that ⟨vN⟩=0 and employing Hölder's inequality, it follows that, for N≥N0=N0(δ),
|⟨fN(uN)⟩|≤cδ‖vN‖‖fN(uN)−⟨fN(uN)⟩‖+c′δ, t∈[0,T0], |
whence
∫T00|⟨fN(uN)⟩|2ds≤cδ‖vN‖2L∞(0,T0;L2(Ω))‖fN(uN)−⟨fN(uN)⟩‖2L2((0,T0)×Ω)+c′δ. | (4.44) |
Therefore, noting that v↦(|⟨v⟩|2+‖v−⟨v⟩‖2)12 is a norm on L2(Ω) which is equivalent to the usual L2-norm, (4.40) and (4.44) yield that
‖fN(uN)‖L2((0,T0)×Ω) | (4.45) |
≤cδ(‖uN‖L∞(0,T0;L2(Ω))+1)(‖uN‖L2(0,T0;H2(Ω))+‖∇μN‖L2((0,T0)×Ω)n)+c′δ. |
Noting finally that ⟨μN⟩=⟨fN(uN)⟩, we deduce that
‖μN‖L2(0,T0;H1(Ω)) | (4.46) |
≤cδ(‖uN‖L∞(0,T0;L2(Ω))+1)(‖uN‖L2(0,T0;H2(Ω))+‖∇μN‖L2((0,T0)×Ω)n)+c′δ. |
Having this, we can now proceed exactly as in Section 2 to pass to the limit and prove the separation property.
Remark 4.3. Actually, a more careful treatment of the equation for the spatial average of the order parameter allows to prove the global in time existence of solutions (see [194]). Indeed, rewriting (4.1) as
∂u∂t+Δ2u−Δf(u)+u−χD(x)u=0, |
we have, integrating this equation over Ω,
d⟨u⟩dt+⟨u⟩=1Vol(Ω)∫Dudx. |
This yields that
⟨u(t)⟩=e−t⟨u0⟩+1Vol(Ω)e−t∫t0esds∫Dudx. |
Then, as long as the solution exists, necessarily, |u(t)|≤1, so that
|⟨u(t)⟩|≤e−t|⟨u0⟩|+Vol(D)Vol(Ω)e−t∫t0esds, |
whence
|⟨u(t)⟩|≤e−t|⟨u0⟩|+Vol(D)Vol(Ω)(1−e−t). |
We now consider the function
φ(t)=e−t|⟨u0⟩|+Vol(D)Vol(Ω)(1−e−t). |
Then,
φ′(t)=(−|⟨u0⟩|+Vol(D)Vol(Ω))e−t. |
If −|⟨u0⟩|+Vol(D)Vol(Ω)≥0, then φ is monotone increasing and
φ(0)≤φ(t)≤limt→+∞φ(t), |
that is,
|⟨u0⟩|≤φ(t)≤Vol(D)Vol(Ω). |
Furthermore, if −|⟨u0⟩|+Vol(D)Vol(Ω)≤0, then φ is monotone decreasing and
limt→+∞φ(t)≤φ(t)≤φ(0), |
that is
Vol(D)Vol(Ω)≤φ(t)≤|⟨u0⟩|. |
It thus follows that
|⟨u(t)⟩|≤max(|⟨u0⟩|,Vol(D)Vol(Ω)), |
whence
|⟨u(t)⟩|≤1−δ, |
where δ=δ(u0)∈(0,1) is independent of time. Therefore, the solutions are indeed global in time.
Remark 4.4. The uniqueness of solutions, as well as further regularity results, are important open problems in the case of logarithmic nonlinear terms and will be addressed in [194].
Remark 4.5. The Cahn–Hilliard inpainting model studied in this section was extended to color images in [75], by considering systems of Cahn–Hilliard equations, and to grayscale images in [76], by considering a complex version of the Cahn–Hilliard inpainting model; see also [41], where systems of Cahn–Hilliard equations were used for grayscale images.
Remark 4.6. As far as the numerical simulations are concerned, the authors in [24,25] proposed a dynamic two-steps algorithm based on the interface thickness ε. More precisely, one first takes a large value of ε in order to join the edges (indeed, when the inpainting domain is large, the inpainting may fail if the interface thickness is too small) and then switches to a smaller value of ε in order to obtain the final restored image. This algorithm is very efficient as far as the computation time and the quality of the restored images are concerned. In [73,74,75], we proposed instead a one-step algorithm with threshold. Namely, we take an intermediate value of ε and then threshold, i.e., when the order parameter is larger than some given value, we take it equal to 1 (say, black) and, when it is smaller, we take it equal to 0 (white); of course, such an algorithm does not make sense for grayscale images. We observed that we can obtain results which are comparable with those in [24,25], when the inpainting domain is not too large, but with a smaller computation time. When the inpainting domain is large, this algorithm may fail, but, as already mentioned, taking logarithmic nonlinear terms instead of polynomial ones, improves the simulations.
The author wishes to thank A. Giorgini for several useful comments.
The author declares no conflicts of interest in this paper.
[1] | H. Abels, On a diffuse interface model for two-phase flows of viscous, incompressible fluids with matched densities, Arch. Ration. Mech. Anal. 194 (2009), 463-506. |
[2] | H. Abels, S. Bosia and M. Grasselli, Cahn-Hilliard equation with nonlocal singular free energies, Ann. Mat. Pura Appl. 194 (2015), 1071-1106. |
[3] | H. Abels and E. Feireisl, On a diffuse interface model for a two-phase flow of compressible viscous fluids, Indiana Univ. Math. J. 57 (2008), 659-698. |
[4] | H. Abels and M. Wilke, Convergence to equilibrium for the Cahn-Hilliard equation with a logarithmic free energy, Nonlinear Anal. 67 (2007), 3176-3193. |
[5] | M. Ainsworth and Z. Mao, Well-posedness of the Cahn-Hilliard equation with fractional free energy and its Fourier Galerkin approximation, Chaos Solitons Fractals 102 (2017), 264-273. |
[6] | M. Ainsworth and Z. Mao, Analysis and approximation of a fractional Cahn-Hilliard equation, SIAM J. Numer. Anal. 55 (2017), 1689-1718. |
[7] | S.M. Allen and J.W. Cahn, A microscopic theory for antiphase boundary motion and its application to antiphase domain coarsening, Acta Metall. 27 (1979), 1085-1095. |
[8] | H.W. Alt and I. Pawłow, A mathematical model of dynamics of non-isothermal phase separation, Physica D 59 (1992), 389-416. |
[9] | H.W. Alt and I. Pawłow, Existence of solutions for non-isothermal phase separation, Adv. Math. Sci. Appl. 1 (1992), 319-409. |
[10] | P.F. Antonietti, L. Beirão da Veiga, S. Scacchi and M. Verani, C1virtual element method for the Cahn-Hilliard equation with polygonal meshes, SIAM J. Numer. Anal. 54 (2016), 34-56. |
[11] | A.R. Appadu, J.K. Djoko, H.H. Gidey and J.M.S. Lubuma, Analysis of multilevel finite volume approximation of 2D convective Cahn-Hilliard equation, Jpn. J. Ind. Appl. Math. 34 (2017), 253-304. |
[12] | P. Areias, E. Samaniego and T. Rabczuk, A staggered approach for the coupling of Cahn-Hilliard type diffusion and finite strain elasticity, Comput. Mech. 57 (2016), 339-351. |
[13] | A. Aristotelous, O. Karakashian and S.M. Wise, A mixed discontinuous Galerkin, convex splitting scheme for a modified Cahn-Hilliard equation and an efficient nonlinear multigrid solver, Discrete Contin. Dyn. Systems Ser. B 18 (2013), 2211-2238. |
[14] | A.C. Aristotelous, O.A. Karakashian and S.M. Wise, Adaptive, second-order in time, primitivevariable discontinuous Galerkin schemes for a Cahn-Hilliard equation with a mass source, IMA J. Numer. Anal. 35 (2015), 1167-1198. |
[15] | A. V. Babin and M. I. Vishik, Attractors of evolution equations, North-Holland, Amsterdam, 1992. |
[16] | F. Bai, C.M. Elliott, A. Gardiner, A. Spence and A.M. Stuart, The viscous Cahn-Hilliard equation. Part Ⅰ: computations, Nonlinearity 8 (1995), 131-160. |
[17] | L. Baňas and R. Nürnberg, A multigrid method for the Cahn-Hilliard equation with obstacle potential, Appl. Math. Comput. 213 (2009), 290-303. |
[18] | J.W. Barrett and J.F. Blowey, An error bound for the finite element approximation of the CahnHilliard equation with logarithmic free energy, Numer. Math. 72 (1995), 257-287. |
[19] | J.W. Barrett and J.F. Blowey, Finite element approximation of the Cahn-Hilliard equation with concentration dependent mobility, Math. Comput. 68 (1999), 487-517. |
[20] | J.W. Barrett, J.F. Blowey and H. Garcke, Finite element approximation of the Cahn-Hilliard equation with degenerate mobility, SIAM J. Numer. Anal. 37 (1999), 286-318 |
[21] | S. Bartels and R. Müller, A posteriori error controlled local resolution of evolving interfaces for generalized Cahn-Hilliard equations, Interfaces Free Bound. 12 (2010), 45-73. |
[22] | S. Bartels and R. Müller, Error control for the approximation of Allen-Cahn and Cahn-Hilliard equations with a logarithmic potential, Numer. Math. 119 (2011), 409-435. |
[23] | P.W. Bates and J. Han, The Neumann boundary problem for a nonlocal Cahn-Hilliard equation, J. Diff. Eqns. 212 (2005), 235-277. |
[24] | A. Bertozzi, S. Esedoglu and A. Gillette, Inpainting of binary images using the Cahn-Hilliard equation, IEEE Trans. Imag. Proc. 16 (2007), 285-291. |
[25] | A. Bertozzi, S. Esedoglu and A. Gillette, Analysis of a two-scale Cahn-Hilliard model for binary image inpainting, Multiscale Model. Simul. 6 (2007), 913-936. |
[26] | K. Binder and H.L. Frisch, Dynamics of surface enrichment: A theory based on the Kawasaki spin-exchange model in the presence of a wall, Z. Phys. B 84 (1991), 403-418. |
[27] | T. Blesgen and I.V. Chenchiah, Cahn-Hilliard equations incorporating elasticity: analysis and comparison to experiments, Philos. Trans. R. Soc. Lond. Ser. A Math. Phys. Eng. Sci. 371 (2013), 1-16. |
[28] | T. Blesgen and A. Schlömerkemper, On the Allen-Cahn/Cahn-Hilliard system with a geometrically linear elastic energy, Proc. Roy. Soc. Edinburgh Sect. A 144 (2014), 241-266. |
[29] | D. Blömker, B. Gawron and T. Wanner, Nucleation in the one-dimensional stochastic CahnHilliard model, Discrete Contin. Dyn. Systems 27 (2010), 25-52. |
[30] | D. Blömker, S. Maier-Paape and T. Wanner, Second phase spinodal decomposition for the CahnHilliard-Cook equation, Trans. Amer. Math. Soc. 360 (2008), 449-489. |
[31] | J.F. Blowey and C.M. Elliott, The Cahn-Hilliard gradient theory for phase separation with nonsmooth free energy. Part Ⅰ. Mathematical analysis, Eur. J. Appl. Math. 2 (1991), 233-280. |
[32] | L. Bo, K. Shi and Y. Wang, Support theorem for a stochastic Cahn-Hilliard equation, Electron. J. Prob. 15 (2010), 484-525. |
[33] | L. Bo and Y. Wang, Stochastic Cahn-Hilliard partial differential equations with Lévy spacetime white noise, Stochastics and Dynamics 6 (2006), 229-244. |
[34] | E. Bonetti, P. Colli, W. Dreyer, G. Gilardi, G. Schimperna and J. Sprekels, On a model for phase separation in binary alloys driven by mechanical effects, Physica D 165 (2002), 48-65. |
[35] | E. Bonetti, W. Dreyer and G. Schimperna, Global solution to a viscous Cahn-Hilliard equation for tin-lead alloys with mechanical stresses, Adv. Diff. Eqns. 2 (2003), 231-256. |
[36] | A. Bonfoh, M. Grasselli and A. Miranville, Long time behavior of a singular perturbation of the viscous Cahn-Hilliard-Gurtin equation, Math. Methods Appl. Sci. 31 (2008), 695-734. |
[37] | A. Bonfoh, M. Grasselli and A. Miranville, Inertial manifolds for a singular perturbation of the viscous Cahn-Hilliard-Gurtin equation, Topol. Methods Nonlinear Anal. 35 (2010), 155-185. |
[38] | A. Bonfoh, M. Grasselli and A. Miranville, Singularly perturbed 1D Cahn-Hilliard equation revisited, Nonlinear Diff. Eqns. Appl. (NoDEA) 17 (2010), 663-695. |
[39] | A. Bonfoh and A. Miranville, On Cahn-Hilliard-Gurtin equations, Nonlinear Anal. 47 (2001), 3455-3466. |
[40] | J. Bosch and M. Stoll, Preconditioning for vector-valued Cahn-Hilliard equations, SIAM J. Sci. Comput. 37 (2015), S216-S243. |
[41] | J. Bosch and M. Stoll, A fractional inpainting model based on the vector-valued Cahn-Hilliard equation, SIAM J. Imaging Sci. 8 (2015), 2352-2382. |
[42] | S. Bosia, M. Conti and M. Grasselli, On the Cahn-Hilliard-Brinkman system, Commun. Math. Sci. 13 (2015), 1541-1567. |
[43] | S. Bosia, M. Grasselli and A. Miranville, On the longtime behavior of a 2D hydrodynamic model for chemically reacting binary fluid mixtures, Math. Methods Appl. Sci. 37 (2014), 726-743. |
[44] | F. Boyer, Nonhomogeneous Cahn-Hilliard fluids, Ann. Inst. H. PoincaréAnal. Non Linéaire 18 (2001), 225-259. |
[45] | F. Boyer, A theoretical and numerical model for the study of incompressible mixture flows, Computers and Fluids 31 (2002), 41-68. |
[46] | F. Boyer, L. Chupin and P. Fabrie, Numerical study of viscoelastic mixtures through a CahnHilliard flow model, Eur. J. Mech. B Fluids 23 (2004), 759-780. |
[47] | F. Boyer and C. Lapuerta, Study of a three component Cahn-Hilliard flow model, M2AN Math. Model. Numer. Anal. 40 (2006), 653-687. |
[48] | F. Boyer, C. Lapuerta, S. Minjeaud and B. Piar, A local adaptive refinement method with multigrid preconditionning illustrated by multiphase flows simulations, ESAIM Proc. 27 (2009), 15-53. |
[49] | F. Boyer, C. Lapuerta, S. Minjeaud, B. Piar and M. Quintard, Cahn-Hilliard/Navier-Stokes model for the simulation of three-phase flows, Transp. Porous Media 82 (2010), 463-483. |
[50] | F. Boyer and S. Minjeaud, Numerical schemes for a three component Cahn-Hilliard model, M2AN Math. Model. Numer. Anal. 45 (2011), 697-738. |
[51] | F. Boyer and S. Minjeaud, Hierarchy of consistent n-component Cahn-Hilliard systems, Math. Models Methods Appl. Sci. 24 (2014), 2885-2928. |
[52] | F. Boyer and F. Nabet, A DDFV method for a Cahn-Hilliard/Stokes phase field model with dynamic boundary conditions, M2AN Math. Model. Numer. Anal. , to appear |
[53] | L.A. Caffarelli and N.E. Muler, An L∞ bound for solutions of the Cahn-Hilliard equation, Arch. Ration. Mech. Anal. 133 (1995), 129-144. |
[54] | G. Caginalp, An analysis of a phase field model of a free boundary, Arch. Ration. Mech. Anal. 92 (1986), 205-245. |
[55] | G. Caginalp and X. Chen, Phase field equations in the singular limit of sharp interface problems, in On the evolution of phase boundaries, IMA Vol. Math. Appl. 43, M. Gurtin ed. , Springer, New York, 1-27,1992. |
[56] | G. Caginalp and X. Chen, Convergence of the phase field model to its sharp interface limits, European J. Appl. Math. 9 (1998), 417-445. |
[57] | G. Caginalp and E. Esenturk, Anisotropic phase field equations of arbitrary order, Discrete Contin. Dyn. Systems Ser. S 4 (2011), 311-350. |
[58] | J.W. Cahn, On spinodal decomposition, Acta Metall. 9 (1961), 795-801. |
[59] | J.W. Cahn, C.M. Elliott and A. Novick-Cohen, The Cahn-Hilliard equation with a concentration dependent mobility: motion by minus the Laplacian of the mean curvature, Eur. J. Appl. Math. 7 (1996), 287-301. |
[60] | J.W. Cahn and J.E. Hilliard, Free energy of a nonuniform system Ⅰ. Interfacial free energy, J. Chem. Phys. 28 (1958), 258-267. |
[61] | C. Cao and C.G. Gal, Global solutions for the 2D NS-CH model for a two-phase flow of viscous, incompressible fluids with mixed partial viscosity and mobility, Nonlinearity 25 (2012), 3211-3234. |
[62] | J.W. Cahn and J.E. Hilliard, Free energy of a nonuniform system Ⅲ. Nucleation in a two component incompressible fluid, J. Chem. Phys. 31 (1959), 688-699. |
[63] | C. Cardon-Weber, Cahn-Hilliard stochastic equation: existence of the solution and of its density, Bernouilli 7 (2001), 777-816. |
[64] | M. Carrive, A. Miranville and A. Piétrus, The Cahn-Hilliard equation for deformable continua, Adv. Math. Sci. Appl. 10 (2000), 539-569. |
[65] | A.N. Carvalho and T. Dlotko, Dynamics of the viscous Cahn-Hilliard equation, J. Math. Anal. Appl. 344 (2008), 703-725. |
[66] | V. Chalupeckí, Numerical studies of Cahn-Hilliard equations and applications in image processing, in Proceedings of Czech-Japanese Seminar in Applied Mathematics 2004 (August 4-7,2004), Czech Technical University in Prague. |
[67] | F. Chave, D.A. Di Pietro, F. Marche and F. Pigeonneau, A hybrid high-order method for the CahnHilliard problem in mixed form, SIAM J. Numer. Anal. 54 (2016), 1873-1898. |
[68] | F. Chen and J. Shen, Efficient energy stable schemes with spectral discretization in space for anisotropic Cahn-Hilliard systems, Commun. Comput. Phys. 13 (2013), 1189-1208. |
[69] | L. Chen and C. Xu, A time splitting space spectral element method for the Cahn-Hilliard equation, East Asian J. Appl. Math. 3 (2013), 333-351. |
[70] | X. Chen, G. Caginalp and E. Esenturk, Interface conditions for a phase field model with anisotropic and non-local interactions, Arch. Rational Mech. Anal. 202 (2011), 349-372. |
[71] | K. Cheng, C. Wang, S.M. Wise and Y. Yue, A second-order, weakly energy-stable pseudo-spectral scheme for the Cahn-Hilliard equation and its solution by the homogeneous linear iteration method, J. Sci. Comput. 69 (2016), 1083-1114. |
[72] | L. Cherfils, H. Fakih, M. Grasselli and A. Miranville, A convergent convex splitting scheme for a nonlocal Cahn-Hilliard-Oono type equation with a transport term, in preparation. |
[73] | L. Cherfils, H. Fakih and A. Miranville, Finite-dimensional attractors for the Bertozzi-EsedogluGillette-Cahn-Hilliard equation in image inpainting, Inv. Prob. Imag. 9 (2015), 105-125. |
[74] | L. Cherfils, H. Fakih and A. Miranville, On the Bertozzi-Esedoglu-Gillette-Cahn-Hilliard equation with logarithmic nonlinear terms, SIAM J. Imag. Sci. 8 (2015), 1123-1140. |
[75] | L. Cherfils, H. Fakih and A. Miranville, A Cahn-Hilliard system with a fidelity term for color image inpainting, J. Math. Imag. Vision 54 (2016), 117-131. |
[76] | L. Cherfils, H. Fakih and A. Miranville, A complex version of the Cahn-Hilliard equation for grayscale image inpainting, Multiscale Model. Simul. 15 (2017), 575-605. |
[77] | L. Cherfils, S. Gatti and Miranville, A variational approach to a Cahn-Hilliard model in a domain with nonpermeable walls, J. Math. Sci. (N.Y.) 189 (2012), 604-636. |
[78] | L. Cherfils, S. Gatti and A. Miranville, Corrigendum to "Existence of global solutions to the Caginalp phase-field system with dynamic boundary conditions and singular potentials"[J. Math. Anal. Appl. 343 (2008), 557-566], J. Math. Anal. Appl. 348 (2008), 1029-1030. |
[79] | L. Cherfils and A. Miranville, Generalized Cahn-Hilliard equations with a logarithmic free energy, Rev. Real Acad. Sci. 94 (2000), 19-32. |
[80] | L. Cherfils and A. Miranville, On the Caginalp system with dynamic boundary conditions and singular potentials, Appl. Math. 54 (2009), 89-115. |
[81] | L. Cherfils, A. Miranville and S. Peng, Higher-order models in phase separation, J. Appl. Anal. Comput. 7 (2017), 39-56. |
[82] | L. Cherfils, A. Miranville and S. Peng, Higher-order anisotropic models in phase separation, Adv. Nonlinear Anal. , to appear. |
[83] | L. Cherfils, A. Miranville, S. Peng and W. Zhang, Higher-order generalized Cahn-Hilliard equations, Electron. J. Qualitative Theory Diff. Eqns. 9 (2017), 1-22. |
[84] | L. Cherfils, A. Miranville and S. Zelik, The Cahn-Hilliard equation with logarithmic potentials, Milan J. Math. 79 (2011), 561-596. |
[85] | L. Cherfils, A. Miranville and S. Zelik, On a generalized Cahn-Hilliard equation with biological applications, Discrete Contin. Dyn. Systems Ser. B 19 (2014), 2013-2026. |
[86] | L. Cherfils and M. Petcu, On the viscous Cahn-Hilliard-Navier-Stokes equations with dynamic boundary conditions, Commun. Pure Appl. Anal. 15 (2016), 1419-1449. |
[87] | L. Cherfils, M. Petcu and M. Pierre, A numerical analysis of the Cahn-Hilliard equation with dynamic boundary conditions, Discrete Contin. Dyn. Systems 27 (2010), 1511-1533. |
[88] | R. Chill, E. Fašangová and J. Prüss, Convergence to steady states of solutions of the Cahn-Hilliard equation with dynamic boundary conditions, Math. Nachr. 279 (2006), 1448-1462. |
[89] | Y. Choi, D. Jeong and J. Kim, A multigrid solution for the Cahn-Hilliard equation on nonuniform grids, Appl. Math. Comput. 293 (2017), 320-333. |
[90] | R. Choksi and X. Ren, On a derivation of a density functional theory for microphase separation of diblock copolymers, J. Statist. Phys. 113 (2003), 151-176. |
[91] | J.W. Cholewa and T. Dlotko, Global attractor for the Cahn-Hilliard system, Bull. Austral. Math. Soc. 49 (1994), 277-293. |
[92] | J. W. Cholewa and T. Dlotko, Global attractors in abstract parabolic problems, London Mathematical Society Lecture Notes Series, Vol. 278, Cambridge University Press, Cambridge, 2000. |
[93] | S.M. Choo and S.K. Chung, Asymtotic behaviour of the viscous Cahn-Hilliard equation, J. Appl. Math. Comput. 11 (2003), 143-154. |
[94] | L. Chupin, An existence result for a mixture of non-newtonian fluids with stress-diffusion using the Cahn-Hilliard formulation, Discrete Contin. Dyn. Systems Ser. B 3 (2003), 45-68. |
[95] | D. Cohen and J.M. Murray, A generalized diffusion model for growth and dispersion in a population, J. Math. Biol. 12 (1981), 237-248. |
[96] | P. Colli, G. Gilardi and D. Hilhorst, On a Cahn-Hilliard type phase field model related to tumor growth, Discrete Contin. Dyn. Systems 35 (2015), 2423-2442. |
[97] | P. Colli, G. Gilardi, P. Krejci and J. Sprekels, A continuous dependence result for a nonstandard system of phase field equations, Math. Methods Appl. Sci. 37 (2014), 1318-1324. |
[98] | P. Colli, G. Gilardi, P. Podio-Guidugli and J. Sprekels, Global existence for a strongly coupled Cahn-Hilliard system with viscosity, Boll. Unione Mat. Ital. 5 (2012), 495-513. |
[99] | P. Colli, G. Gilardi, P. Podio-Guidugli and J. Sprekels, An asymptotic analysis for a nonstandard Cahn-Hilliard system with viscosity, Discrete Contin. Dyn. Systems Ser. S 6 (2013), 353-368. |
[100] | P. Colli, G. Gilardi, P. Podio-Guidugli and J. Sprekels, Global existence and uniqueness for a singular/degenerate Cahn-Hilliard system with viscosity, J. Diff. Eqns. 254 (2013), 4217-4244. |
[101] | P. Colli, G. Gilardi, E. Rocca and J. Sprekels, Vanishing viscosities and error estimate for a CahnHilliard type phase-field system related to tumor growth, Nonlinear Anal. Real World Appl. 26 (2015), 93-108. |
[102] | P. Colli, G. Gilardi, E. Rocca and J. Sprekels, Asymptotic analyses and error estimates for a CahnHilliard type phase field system modelling tumor growth, Discrete Contin. Dyn. Systems Ser. S 10 (2017), 37-54. |
[103] | P. Colli, G. Gilardi, E. Rocca and J. Sprekels, Optimal distributed control of a diffuse interface model of tumor growth, Nonlinearity 30 (2017), 2518-2546. |
[104] | P. Colli, G. Gilardi and J. Sprekels, On the Cahn-Hilliard equation with dynamic boundary conditions and a dominating boundary potential, J. Math. Anal. Appl. 419 (2014), 972-994. |
[105] | P. Colli, G. Gilardi and J. Sprekels, Global existence for a nonstandard viscous Cahn-Hilliard system with dynamic boundary condition, SIAM J. Math. Anal. 49 (2017), 1732-1760. |
[106] | M. Conti and M. Coti Zelati, Attractors for the Cahn-Hilliard equation with memory in 2D, Nonlinear Anal. 72 (2010), 1668-1682. |
[107] | M. Conti, S. Gatti and A. Miranville, Multi-component Cahn-Hilliard systems with dynamic boundary conditions, Nonlinear Anal. Real World Appl. 25 (2015), 137-166. |
[108] | M. Conti and A. Giorgini, On the Cahn-Hilliard-Brinkman system with singular potential and nonconstant viscosity, submitted. |
[109] | M. Conti and G. Mola, 3-D viscous Cahn-Hilliard equation with memory, Math. Methods Appl. Sci. 32 (2009), 1370-1395. |
[110] | H. Cook, Brownian motion in spinodal decomposition, Acta Metall. 18 (1970), 297-306. |
[111] | M.I.M. Copetti and C.M. Elliott, Numerical analysis of the Cahn-Hilliard equation with a logarithmic free energy, Numer. Math. 63 (1992), 39-65. |
[112] | G. Da Prato and A. Debussche, Stochastic Cahn-Hilliard equation, Nonlinear Anal. 26 (1996), 241-263. |
[113] | M. Dai, E. Feireisl, E. Rocca, G. Schimperna and M.E. Schonbek, Analysis of a diffuse interface model of multispecies tumor growth, Nonlinearity 30 (2017), 1639-1658. |
[114] | R. Dal Passo, L. Giacomelli and A. Novick-Cohen, Existence for an Allen-Cahn/Cahn-Hilliard system with degenerate mobility, Interfaces Free Bound. 1 (1999), 199-226. |
[115] | P.G. de Gennes, Dynamics of fluctuations and spinodal decomposition in polymer blends, J. Chem. Phys. 72 (1980), 4756-4763. |
[116] | A. Debussche and L. Dettori, On the Cahn-Hilliard equation with a logarithmic free energy, Nonlinear Anal. 24 (1995), 1491-1514. |
[117] | A. Debussche and L. Goudenège, Stochastic Cahn-Hilliard equation with double singular nonlinearities and two reflections, SIAM J. Math. Anal. 43 (2011), 1473-1494. |
[118] | A. Debussche and L. Zambotti, Conservative stochastic Cahn-Hilliard equation with reflection, Ann. Probab. 35 (2007), 1706-1739. |
[119] | F. Della Porta, A. Giorgini and M. Grasselli, The nonlocal Cahn-Hilliard-Hele-Shaw system with singular potential, submited. |
[120] | F. Della Porta and M. Grasselli, On the nonlocal Cahn-Hilliard-Brinkman and Cahn-HilliardHele-Shaw systems, Commun. Pure Appl. Anal. 15 (2016), 299-317. Erratum, Commun. Pure Appl. Anal. 16 (2017), 369-372. |
[121] | C.V. Di Leo, E. Rejovitzky and L. Anand, A Cahn-Hilliard-type phase-field theory for species diffusion coupled with large elastic deformations: application to phase-separating Li-ion electrode materials, J. Mech. Phys. Solids 70 (2014), 1-29. |
[122] | A. Diegel, C. Wang and S.M. Wise, Stability and convergence of a second order mixed finite element method for the Cahn-Hilliard equation, IMA J. Numer. Anal. 36 (2016), 1867-1897. |
[123] | T. Dlotko, Global attractor for the Cahn-Hilliard equation in H2 and H3, J. Diff. Eqns. 113 (1994), 381-393. |
[124] | I.C. Dolcetta and S.F. Vita, Area-preserving curve-shortening flows: from phase separation to image processing, Interfaces Free Bound. 4 (2002), 325-343. |
[125] | A. Eden, C. Foias, B. Nicolaenko and R. Temam, Exponential attractors for dissipative evolution equations, Research in Applied Mathematics, Vol. 37, John-Wiley, New York, 1994. |
[126] | A. Eden and V.K. Kalantarov, The convective Cahn-Hilliard equation, Appl. Math. Lett. 20 (2007), 455-461. |
[127] | A. Eden and V.K. Kalantarov, 3D convective Cahn-Hilliard equation, Commun. Pure Appl. Anal. 6 (2007), 1075-1086. |
[128] | A. Eden, V. Kalantarov and S.V. Zelik, Global solvability and blow up for the convective CahnHilliard equations with concave potentials, J. Math. Phys. 54 (2013), 1-12. |
[129] | A. Eden, V. Kalantarov and S.V. Zelik, Infinite energy solutions for the Cahn-Hilliard equation in cylindrical domains, Math. Methods Appl. Sci. 37 (2014), 1884-1908. |
[130] | M. Efendiev, H. Gajewski and S. Zelik, The finite dimensional attractor for a 4th order system of the Cahn-Hilliard type with a supercritical nonlinearity, Adv. Diff. Eqns. 7 (2002), 1073-1100. |
[131] | M. Efendiev and A. Miranville, New models of Cahn-Hilliard-Gurtin equations, Contin. Mech. Thermodyn. 16 (2004), 441-451. |
[132] | M. Efendiev, A. Miranville and S. Zelik, Exponential attractors for a singularly perturbed CahnHilliard system, Math. Nach. 272 (2004), 11-31. |
[133] | N. Elezovic and A. Mikelic, On the stochastic Cahn-Hilliard equation, Nonlinear Anal. 16 (1991), 1169-1200. |
[134] | C. M. Elliott, The Cahn-Hilliard model for the kinetics of phase separation, in Mathematical models for phase change problems, J. F. Rodrigues ed. , International Series of Numerical Mathematics, Vol. 88, Birkhauser, Bäsel, 1989. |
[135] | C.M. Elliott and D.A. French, Numerical studies of the Cahn-Hilliard equation for phase separation, IMA J. Appl. Math. 38 (1987), 97-128. |
[136] | C.M. Elliott and D.A. French, A non-conforming finite element method for the two-dimensional Cahn-Hilliard equation, SIAM J. Numer. Anal. 26 (1989), 884-903. |
[137] | C.M. Elliott, D.A. French and F.A. Milner, A second order splitting method for the Cahn-Hilliard equation, Numer. Math. 54 (1989), 575-590. |
[138] | C.M. Elliott and H. Garcke, On the Cahn-Hilliard equation with degenerate mobility, SIAM J. Math. Anal. 27 (1996), 404-423. |
[139] | C.M. Elliott and H. Garcke, Diffusional phase transitions in multicomponent systems with a concentration dependent mobility matrix, Physica D 109 (1997), 242-256. |
[140] | C. M. Elliott and S. Luckhaus, A generalized diffusion equation for phase separation of a multicomponent mixture with interfacial energy, SFB 256 Preprint No. 195, University of Bonn, 1991. |
[141] | C.M. Elliott and T. Ranner, Evolving surface finite element method for the Cahn-Hilliard equation, Numer. Math. 129 (2015), 483-534. |
[142] | C.M. Elliott and A.M. Stuart, Viscous Cahn-Hilliard equation Ⅱ. Analysis, J. Diff. Eqns. 128 (1996), 387-414. |
[143] | C.M. Elliott and S. Zheng, On the Cahn-Hilliard equation, Arch. Ration. Mech. Anal. 96 (1986), 339-357. |
[144] | H. Emmerich, H. Löwen, R. Wittkowski, T. Gruhn, G.I. Tóth, G. Tegze and L. Gránásy, Phasefield-crystal models for condensed matter dynamics on atomic length and diffusive time scales: an overview, Adv. Phys. 61 (2012), 665-743. |
[145] | J. Erlebacher, M.J. Aziz, A. Karma, N. Dimitrov and K. Sieradzki, Evolution of nanoporosity in dealloying, Nature 410 (2001), 450-453. |
[146] | J.D. Eyre, Systems of Cahn-Hilliard equations, SIAM J. Appl. Math. 53 (1993), 1686-1712. |
[147] | J. D. Eyre, Unconditionally gradient stable time marching the Cahn-Hilliard equation, in Computational and mathematical models of microstructural evolution, J. W. Bullard, R. Kalia, M. Stoneham and L. Q. Chen eds. , The Materials Research Society, 1998. |
[148] | H. Fakih, A Cahn-Hilliard equation with a proliferation term for biological and chemical applications, Asymptot. Anal. 94 (2015), 71-104. |
[149] | H. Fakih, Asymptotic behavior of a generalized Cahn-Hilliard equation with a mass source, Appl. Anal. 96 (2017), 324-348. |
[150] | X. Feng, Y. Li and Y. Xing, Analysis of mixed interior penalty discontinuous Galerkin methods for the Cahn-Hilliard equation and the Hele-Shaw flow, SIAM J. Numer. Anal. 54 (2016), 825-847. |
[151] | X. Feng and A. Prohl, Error analysis of a mixed finite element method for the Cahn-Hilliard equation, Numer. Math. 99 (2004), 47-84. |
[152] | X. Feng and A. Prohl, Numerical analysis of the Cahn-Hilliard equation and approximation for the Hele-Shaw problem, Interfaces Free bound. 7 (2005), 1-28. |
[153] | X. Feng and S. Wise, Analysis of a Darcy-Cahn-Hilliard diffuse interface model for the HeleShaw flow and its fully discrete finite element approximation, SIAM J. Numer. Anal. 50 (2012), 1320-1343. |
[154] | W.M. Feng, P. Yu, S.Y. Hu, Z.K. Liu, Q. Du and L.Q. Chen, A Fourier spectral moving mesh method for the Cahn-Hilliard equation with elasticity, Commun. Comput. Phys. 5 (2009), 582-599. |
[155] | H.P. Fischer, P. Maass and W. Dieterich, Novel surface modes in spinodal decomposition, Phys. Rev. Lett. 79 (1997), 893-896. |
[156] | H.P. Fischer, P. Maass and W. Dieterich, Diverging time and length scales of spinodal decomposition modes in thin flows, Europhys. Lett. 42 (1998), 49-54. |
[157] | H.P. Fischer, J. Reinhard, W. Dieterich, J.-F. Gouyet, P. Maass, A. Majhofer and D. Reinel, Timedependent density functional theory and the kinetics of lattice gas systems in contact with a wall, J. Chem. Phys. 108 (1998), 3028-3037. |
[158] | S. Frigeri and M. Grasselli, Nonlocal Cahn-Hilliard-Navier-Stokes systems with singular potentials, Dyn. Partial Diff. Eqns. 9 (2012), 273-304. |
[159] | S. Frigeri, M. Grasselli and E. Rocca, On a diffuse interface model of tumor growth, European J. Appl. Math. 26 (2015), 215-243. |
[160] | T. Fukao, S. Yoshikawa and S. Wada, Structure-preserving finite difference schemes for the CahnHilliard equation with dynamic boundary conditions in the one-dimensional case, Commun. Pure Appl. Anal. 16 (2017), 1915-1938. |
[161] | D. Furihata, A stable and conservative finite difference scheme for the Cahn-Hilliard equation, Numer. Math. 87 (2001), 675-699. |
[162] | H. Gajewski and K. Zacharias, On a nonlocal phase separation model, J. Math. Anal. Appl. 286 (2003), 11-31. |
[163] | C.G. Gal, A Cahn-Hilliard model in bounded domains with permeable walls, Math. Methods Appl. Sci. 29 (2006), 2009-2036. |
[164] | C.G. Gal, Exponential attractors for a Cahn-Hilliard model in bounded domains with permeable walls, Electron. J. Diff. Eqns. 2006 (2006), 1-23. |
[165] | C.G. Gal, A. Giorgini and M. Grasselli, The nonlocal Cahn-Hilliard equation with singular potential: well-posedness, regularity and strict separation property, J. Diff. Eqns. 263 (2017), 5253-5297. |
[166] | C.G. Gal and M. Grasselli, Asymptotic behavior of a Cahn-Hilliard-Navier-Stokes system in 2D, Ann. Inst. H. Poincaré Anal. Non Linéaire 27 (2010), 401-436. |
[167] | C.G. Gal and M. Grasselli, Longtime behavior for a model of homogeneous incompressible twophase flows, Discrete Contin. Dyn. Systems 28 (2010), 1-39. |
[168] | C.G. Gal and M. Grasselli, Longtime behavior of nonlocal Cahn-Hilliard equations, Discrete Contin. Dyn. Systems 34 (2014), 145-179. |
[169] | C.G. Gal, M. Grasselli and A. Miranville, Cahn-Hilliard-Navier-Stokes systems with moving contact lines, Calc. Var. Partial Diff. Eqns. 55 (2016), 1-47. |
[170] | C.G. Gal and A. Miranville, Uniform global attractors for non-isothermal viscous and non-viscous Cahn-Hilliard equations with dynamic boundary conditions, Nonlinear Anal. Real World Appl. 10 (2009), 1738-1766. |
[171] | C.G. Gal and A. Miranville, Robust exponential attractors and convergence to equilibria for nonisothermal Cahn-Hilliard equations with dynamic boundary conditions, Discrete Contin. Dyn. Systems Ser. S 2 (2009), 113-147. |
[172] | C.G. Gal and H. Wu, Asymptotic behavior of a Cahn-Hilliard equation with Wentzell boundary conditions and mass conservation, Discrete Contin. Dyn. Systems 22 (2008), 1041-1063. |
[173] | P. Galenko, D. Danilov and V. Lebedev, Phase-field-crystal and Swift-Hohenberg equations with fast dynamics, Phys. Rev. E 79 (2009), 051110. |
[174] | P. Galenko and D. Jou, Kinetic contribution to the fast spinodal decomposition controlled by diffusion, Physica A 388 (2009), 3113-3123. |
[175] | P. Galenko and V. Lebedev, Analysis of the dispersion relation in spinodal decomposition of a binary system, Philos. Mag. Lett. 87 (2007), 821-827. |
[176] | P. Galenko and V. Lebedev, Local nonequilibrium effect on spinodal decomposition in a binary system, Int. J. Thermodyn. 11 (2008), 21-28. |
[177] | P. Galenko and V. Lebedev, Nonequilibrium effects in spinodal decomposition of a binary system, Phys. Lett. A 372 (2008), 985-989. |
[178] | W. Gao and J. Yin, System of Cahn-Hilliard equations with nonconstant interaction matrix, Chinese Ann. Math., Ser. A 20 (1999), 169-176. |
[179] | H. Garcke, On Cahn-Hilliard systems with elasticity, Proc. Roy. Soc. Edinburgh A 133 (2003), 307-331. |
[180] | H. Garcke, On a Cahn-Hilliard model for phase separation with elastic misfit, Ann. Inst. H. Poincare Anal. Non Linéaire 22 (2005), 165-185. |
[181] | H. Garcke, Mechanical effects in the Cahn-Hilliard model: A review on mathematical results, in Mathematical methods and models in phase transitions, A. Miranville ed. , Nova Sci. Publ. , New York, 43-77,2005. |
[182] | H. Garcke, K.F. Lam, E. Sitka and V. Styles, A Cahn-Hilliard-Darcy model for tumour growth with chemotaxis and active transport, Math. Models Methods Appl. Sci. 26 (2016), 1095-1148. |
[183] | H. Garcke and U. Weikard, Numerical approximation of the Cahn-Larché equation, Numer. Math. 100 (2005), 639-662. |
[184] | S. Gatti, M. Grasselli, A. Miranville and V. Pata, On the hyperbolic relaxation of the onedimensional Cahn-Hilliard equation, J. Math. Anal. Appl. 312 (2005), 230-247. |
[185] | S. Gatti, M. Grasselli, A. Miranville and V. Pata, Hyperbolic relaxation of the viscous CahnHilliard equation in 3-D, Math. Models Methods Appl. Sci. 15 (2005), 165-198. |
[186] | S. Gatti, M. Grasselli, A. Miranville and V. Pata, Memory relaxation of first order evolution equations, Nonlinearity 18 (2005), 1859-1883. |
[187] | S. Gatti, M. Grasselli, A. Miranville and V. Pata, Memory relaxation of the one-dimensional CahnHilliard equation, in Dissipative phase transitions, Ser. Adv. Math. Appl. Sci. , Vol. 71, World Sci. Publ. , Hackensack, NJ, 101-114,2006. |
[188] | G. Giacomin and J.L. Lebowitz, Phase segregation dynamics in particle systems with long range interaction Ⅰ. Macroscopic limits, J. Statist. Phys. 87 (1997), 37-61. |
[189] | G. Giacomin and J.L. Lebowitz, Phase segregation dynamics in particle systems with long range interaction Ⅱ. Interface motion, SIAM J. Appl. Math. 58 (1998), 1707-1729. |
[190] | G. Gilardi, A. Miranville and G. Schimperna, On the Cahn-Hilliard equation with irregular potentials and dynamic boundary conditions, Commun. Pure Appl. Anal. 8 (2009), 881-912. |
[191] | G. Gilardi, A. Miranville and G. Schimperna, Long time behavior of the Cahn-Hilliard equation with irregular potentials and dynamic boundary conditions, Chinese Ann. Math., Ser. B 31 (2010), 679-712. |
[192] | A. Giorgini, M. Grasselli and A. Miranville, The Cahn-Hilliard-Oono equation with singular potential, Math. Models Methods Appl. Sci. , to appear. |
[193] | A. Giorgini, M. Grasselli and H. Wu, The Cahn-Hilliard-Hele-Shaw system with singular potential, submitted. |
[194] | A. Giorgini and A. Miranville, On the Cahn-Hilliard equation with fidelity term and singular potential, in preparation. |
[195] | A. Giorgini, A. Miranville and R. Temam, Uniqueness and regularity results for the Navier-StokesCahn-Hilliard-Oono system with singular potentials, submitted. |
[196] | G.R. Goldstein and A. Miranville, A Cahn-Hilliard-Gurtin model with dynamic boundary conditions, Discrete Contin. Dyn. Systems Ser. S 6 (2013), 387-400. |
[197] | G.R. Goldstein, A. Miranville and G. Schimperna, A Cahn-Hilliard model in a domain with nonpermeable walls, Physica D 240 (2011), 754-766. |
[198] | A.A. Golovin, A.A. Nepomnyashchy, S.H. Davis and M.A. Zaks, Convective Cahn-Hilliard models: from coarsening to roughening, Phys. Rev. Lett. 86 (2001), 1550-1553. |
[199] | H. Gomez, V.M. Calo, Y. Basilevs and T.J.R. Hughes, Isogeometric analysis of Cahn-Hilliard phase field model, Comput. Methods Appl. Mech. Engrg. 197 (2008), 4333-4352. |
[200] | G. Gompper and M. Kraus, Ginzburg-Landau theory of ternary amphiphilic systems. I. Gaussian interface fluctuations, Phys. Rev. E 47 (1993), 4289-4300. |
[201] | G. Gompper and M. Kraus, Ginzburg-Landau theory of ternary amphiphilic systems. Ⅱ. Monte Carlo simulations, Phys. Rev. E 47 (1993), 4301-4312. |
[202] | L. Goudenège, Stochastic Cahn-Hilliard equation with singular nonlinearity and reflection, Stochastic Process. Appl. 119 (2009), 3516-3548. |
[203] | L. Goudenège and L. Manca, Asymptotic properties of stochastic Cahn-Hilliard equation with singular nonlinearity and degenerate noise, Stochastic Process. Appl. 125 (2015), 3785-3800. |
[204] | L. Goudenège, D. Martin and G. Vial, High order finite element calculations for the deterministic Cahn-Hilliard equation, J. Sci. Comput. 52 (2012), 294-321. |
[205] | C. Gräser, R. Kornhuber and U. Sack, Nonsmooth Schur-Newton methods for multicomponent Cahn-Hilliard systems, IMA J. Numer. Anal. 35 (2015), 652-679. |
[206] | M. Grasselli, A. Miranville, R. Rossi and G. Schimperna, Analysis of the Cahn-Hilliard equation with a chemical potential dependent mobility, Commun. Partial Diff. Eqns. 36 (2011), 1193-1238. |
[207] | M. Grasselli and M. Pierre, A splitting method for the Cahn-Hilliard equation with inertial term, Math. Models Methods Appl. Sci. 20 (2010), 1-28. |
[208] | M. Grasselli and M. Pierre, Energy stable and convergent finite element schemes for the modified phase field crystal equation, ESAIM Math. Model. Numer. Anal. 50 (2016), 1523-1560. |
[209] | M. Grasselli, G. Schimperna and A. Miranville, The Caginalp phase-field system with coupled dynamic boundary conditions and singular potentials, Discrete Contin. Dyn. Systems 28 (2010), 67-98. |
[210] | M. Grasselli, G. Schimperna, A. Segatti and S. Zelik, On the 3D Cahn-Hilliard equation with inertial term, J. Evol. Eqns. 9 (2009), 371-404. |
[211] | M. Grasselli, G. Schimperna and S. Zelik, On the 2D Cahn-Hilliard equation with inertial term, Commun. Partial Diff. Eqns. 34 (2009), 137-170. |
[212] | M. Grasselli, G. Schimperna and S. Zelik, Trajectory and smooth attractors for Cahn-Hilliard equations with inertial term, Nonlinearity 23 (2010), 707-737. |
[213] | M. Grasselli and H. Wu, Well-posedness and longtime behavior for the modified phase-field crystal equation, Math. Models Methods Appl. Sci. 24 (2014), 2743-2783. |
[214] | M. Grasselli and H. Wu, Robust exponential attractors for the modified phase-field crystal equation, Discrete Contin. Dyn. Systems 35 (2015), 2539-2564. |
[215] | Z. Guan, V. Heinonen, J.S. Lowengrub, C. Wang and S.M. Wise, An energy stable, hexagonal finite difference scheme for the 2D phase field crystal amplitude equations, J. Comput. Phys. 321 (2016), 1026-1054. |
[216] | Z. Guan, J. S. Lowengrub and C. Wang, Convergence analysis for second order accurate convex splitting schemes for the periodic nonlocal Allen-Cahn and Cahn-Hilliard equations, submitted. |
[217] | Z. Guan, J.S. Lowengrub, C. Wang and S.M. Wise, Second-order convex splitting schemes for periodic nonlocal Cahn-Hilliard and Allen-Cahn equations, J. Comput. Phys. 277 (2014), 48-71. |
[218] | Z. Guan, C. Wang and S.M. Wise, A Convergent convex splitting scheme for the periodic nonlocal Cahn-Hilliard equation, Numer. Math. 128 (2014), 377-406. |
[219] | B. Guo, G. Wang and S. Wang, Well posedness for the stochastic Cahn-Hilliard equation driven by Lévy space-time white noise, Diff. Int. Eqns. 22 (2009), 543-560. |
[220] | J. Guo, C. Wang, S.M. Wise and X. Yue, An H2 convergence of a second-order convex-splitting, finite difference scheme for the three-dimensional Cahn-Hilliard equation, Comm. Math. Sci. 14 (2016), 489-515. |
[221] | M. Gurtin, Generalized Ginzburg-Landau and Cahn-Hilliard equations based on a microforce balance, Physica D 92 (1996), 178-192. |
[222] | M. Gurtin, D. Polignone and J. Vinals, Two-phase binary fluids and immiscible fluids described by an order parameter, Math. Models Methods Appl. Sci. 6 (1996), 815-831. |
[223] | D. Han, A decoupled unconditionally stable numerical scheme for the Cahn-Hilliard-Hele-Shaw system, J. Sci. Comput. 66 (2016), 1102-1121. |
[224] | D. Han and X. Wang, Decoupled energy-law preserving numerical schemes for the Cahn-HilliardDarcy system, Numer. Methods Partial Diff. Eqns. 32 (2016), 936-954. |
[225] | D. Han, X. Wang and H. Wu, Existence and uniqueness of global weak solutions to a CahnHilliard-Stokes-Darcy system for two phase incompressible flows in karstic geometry, J. Diff. Eqns. 257 (2014), 3887-3933. |
[226] | L. He and Y. Liu, A class of stable spectral methods for the Cahn-Hilliard equation, J. Comput. Phys. 228 (2009), 5101-5110. |
[227] | Z. Hu, S.M. Wise, C. Wang and J.S. Lowengrub, Stable finite difference, nonlinear multigrid simulation of the phase field crystal equation, J. Comput. Phys. 228 (2009), 5323-5339. |
[228] | Y. Huo, X. Jiang, H. Zhang and Y. Yang, Hydrodynamic effects on phase separation of binary mixtures with reversible chemical reaction, J. Chem. Phys. 118 (2003), 9830-9837. |
[229] | Y. Huo, H. Zhang and Y. Yang, Effects of reversible chemical reaction on morphology and domain growth of phase separating binary mixtures with viscosity difference, Macromolecular Theory Simul. 13 (2004), 280-289. |
[230] | S. Injrou and M. Pierre, Stable discretizations of the Cahn-Hilliard-Gurtin equations, Discrete Contin. Dyn. Systems 22 (2008), 1065-1080. |
[231] | S. Injrou and M. Pierre, Error estimates for a finite element discretization of the Cahn-HilliardGurtin equations, Diff. Int. Eqns. 15 (2010), 1161-1192. |
[232] | H. Israel, Long time behavior of an Allen-Cahn type equation with a singular potential and dynamic boundary conditions, J. Appl. Anal. Comput. 2 (2012), 29-56. |
[233] | H. Israel, Well-posedness and long time behavior of an Allen-Cahn type equation, Commun. Pure Appl. Anal. 12 (2013), 2811-2827. |
[234] | H. Israel, A. Miranville and M. Petcu, Well-posedness and long time behavior of a perturbed Cahn-Hilliard system with regular potentials, Asymptot. Anal. 84 (2013), 147-179. |
[235] | H. Israel, A. Miranville and M. Petcu, Numerical analysis of a Cahn-Hilliard type equation with dynamic boundary conditions, Ric. Mat. 64 (2015), 25-50. |
[236] | D. Jacquemin, Calculation of two phase Navier-Stokes flows using phase-field modeling, J. Comput. Phys. 155 (1999), 96-127. |
[237] | J. Jiang, H. Wu and S. Zheng, Well-posedness and long-time behavior of a nonautonomous CahnHilliard-Darcy system with mass source modeling tumor growth, J. Diff. Eqns. 259 (2015), 3032-3077. |
[238] | G. Karali, and A. Katsoulakis, The role of multiple microscopic mechanisms in cluster interface evolution, J. Diff. Eqns. 235 (2007), 418-438. |
[239] | G. Karali and Y. Nagase, On the existence of solution for a Cahn-Hilliard/Allen-Cahn equation, Discrete Contin. Dyn. Systems Ser. S 7 (2014), 127-137. |
[240] | G. Karali and T. Ricciardi, On the convergence of a fourth order evolution equation to the AllenCahn equation, Nonlinear Anal. 72 (2010), 4271-4281. |
[241] | A. Katsoulakis and G. Vlachos, From microscopic interactions to macroscopic laws of cluster evolution, Phys. Rev., 84 (2000), 1511-1514. |
[242] | D. Kay, V. Styles and E. Süli, Discontinuous Galerkin finite element approximation of the CahnHilliard equation with convection, SIAM J. Numer. Anal. 47 (2009), 2660-2685. |
[243] | D. Kay, V. Styles and R. Welford, Finite element approximation of a Cahn-Hilliard-Navier-Stokes system, Interfaces Free Bound. 10 (2008), 15-43. |
[244] | E. Khain and L.M. Sander, A generalized Cahn-Hilliard equation for biological applications, Phys. Rev. E 77 (2008), 051129. |
[245] | N. Kenmochi, M. Niezgódka and I. Pawłow, Subdifferential operator approach to the CahnHilliard equation with constraint, J. Diff. Eqns. 117 (1995), 320-356. |
[246] | R. Kenzler, F. Eurich, P. Maass, B. Rinn, J. Schropp, E. Bohl and W. Dieterich, Phase separation in confined geometries: solving the Cahn-Hilliard equation with generic boundary conditions, Comput. Phys. Commun. 133 (2001), 139-157. |
[247] | J. Kim, Phase field computations for ternary fluid flows, Comput. Methods Appl. Mech. Engrg. 196 (2007), 4779-4788. |
[248] | J. Kim, Three-dimensional numerical simulations of a phase-field model for anisotropic interfacial energy, Commun. Korean Math. Soc. 22 (2007), 453-464. |
[249] | J. Kim, A numerical method for the Cahn-Hilliard equation with a variable mobility, Commun. Nonlinear Sci. Numer. Simul. 12 (2007), 1560-1571. |
[250] | J. Kim, A generalized continuous surface tension force formulation for phase-field models for multi-component immiscible fluid flows, Comput. Methods Appl. Mech. Engrg. 198 (2009), 37-40. |
[251] | J. Kim and K. Kang, A numerical method for the ternary Cahn-Hilliard system with a degenerate mobility, Appl. Numer. Math 59 (2009), 1029-1042. |
[252] | J. Kim and J. Lowengrub, Phase field modeling and simulation of three-phase flows, Interfaces Free Bound. 7 (2005), 435-466. |
[253] | I. Klapper and J. Dockery, Role of cohesion in the material description of biofilms, Phys. Rev. E 74 (2006), 0319021-0319028. |
[254] | R. Kobayashi, Modelling and numerical simulations of dendritic crystal growth, Phys. D 63 (1993), 410-423. |
[255] | R.V. Kohn and F. Otto, Upper bounds for coarsening rates, Commun. Math. Phys. 229 (2002), 375-395. |
[256] | M. Korzec, P. Nayar and P. Rybka, Global weak solutions to a sixth order Cahn-Hilliard type equation, SIAM J. Math. Anal. 44 (2012), 3369-3387. |
[257] | M. Korzec and P. Rybka, On a higher order convective Cahn-Hilliard type equation, SIAM J. Appl. Math. 72 (2012), 1343-1360. |
[258] | A. Kostianko and S. Zelik, Inertial manifolds for the 3D Cahn-Hilliard equations with periodic boundary conditions, Commun. Pure Appl. Anal. 14 (2015), 2069-2094. |
[259] | J.S. Langer, Theory of spinodal decomposition in alloys, Ann. Phys. 65 (1975), 53-86. |
[260] | N. Lecoq, H. Zapolsky and P. Galenko, Evolution of the structure factor in a hyperbolic model of spinodal decomposition, Eur. Phys. J. Special Topics 177 (2009), 165-175. |
[261] | H.G. Lee and J. Kim, A second-order accurate non-linear difference scheme for the N-component Cahn-Hilliard system, Physica A 387 (2008), 19-20. |
[262] | S. Lee, C. Lee, H.G. Lee and J. Kim, Comparison of different numerical schemes for the CahnHilliard equation, J. Korean Soc. Ind. Appl. Math. 17 (2013), 197-207. |
[263] | D. Li and Z. Qiao, On second order semi-implicit Fourier spectral methods for 2D Cahn-Hilliard equations, J. Sci. Comput. 70 (2017), 301-341. |
[264] | D. Li and C. Zhong, Global attractor for the Cahn-Hilliard system with fast growing nonlinearity, J. Diff. Eqns. 149 (1998), 191-210. |
[265] | Y. Li, J. Kim and N. Wang, An unconditionally energy-stable second-order time-accurate scheme for the Cahn-Hilliard equation on surfaces, Commun. Nonlinear Sci. Numer. Simul. 53 (2017), 213-227. |
[266] | Y. Li, H.G. Lee, B. Xia and J. Kim, A compact fourth-order finite difference scheme for the threedimensional Cahn-Hilliard equation, Comput. Phys. Commun. 200 (2016), 108-116. |
[267] | C. Liu, Convective Cahn-Hilliard equation with degenerate mobility, Dyn. Contin. Discrete Impuls. Systems Ser. A Math. Anal. 16 (2009), 15-25. |
[268] | C. Liu and J. Shen, A phase field model for the mixture of two incompressible fluids and its approximation by a Fourier-spectral method, Physica D 179 (2003), 211-228. |
[269] | C. Liu and H. Tang, Existence of periodic solution for a Cahn-Hilliard/Allen-Cahn equation in two space dimensions, Evol. Eqns. Control Theory 6 (2017), 219-237. |
[270] | F. Liu and J. Shen, Stabilized semi-implicit spectral deferred correction methods for Allen-Cahn and Cahn-Hilliard equations, Math. Methods Appl. Sci. 38 (2015), 4564-4575. |
[271] | Q. -X. Liu, A. Doelman, V. Rottschäfer, M. de Jager, P. M. J. Herman, M. Rietkerk and J. van de Koppel, Phase separation explains a new class of self-organized spatial patterns in ecological systems, Proc. Nation. Acad. Sci. , http://www.pnas.org/cgi/doi/10.1073/pnas.1222339110. |
[272] | J. Lowengrub, E. Titi and K. Zhao, Analysis of a mixture model of tumor growth, European J. Appl. Math. 24 (2013), 691-734. |
[273] | J. Lowengrub and L. Truskinovski, Quasi-incompressible Cahn-Hilliard fluids and topological transitions, Proc. Royal Soc. London Ser. A 454 (1998), 2617-2654. |
[274] | T. Ma and S. Wang, Cahn-Hilliard equations and phase transition dynamics for binary systems, Discrete Contin. Dyn. Systems 11 (2009), 741-784. |
[275] | S. Maier-Paape, K. Mischaikow and T. Wanner, Rigorous numerics for the Cahn-Hilliard equation on the unit square, Rev. Mat. Complutense 21 (2008), 351-426. |
[276] | S. Maier-Paape and T. Wanner, Spinodal decomposition for the Cahn-Hilliard equation in higher dimensions. Part Ⅰ: Probability and wavelength estimate, Commun. Math. Phys. 195 (1998), 435-464. |
[277] | S. Maier-Paape and T. Wanner, Spinodal decomposition for the Cahn-Hilliard equation in higher dimensions: Nonlinear dynamics, Arch. Ration. Mech. Anal. 151 (2000), 187-219. |
[278] | A. Makki and A. Miranville, Well-posedness for one-dimensional anisotropic Cahn-Hilliard and Allen-Cahn systems, Electron. J. Diff. Eqns. 2015 (2015), 1-15. |
[279] | A. Makki and A. Miranville, Existence of solutions for anisotropic Cahn-Hilliard and Allen-Cahn systems in higher space dimensions, Discrete Contin. Dyn. Systems Ser. S 9 (2016), 759-775. |
[280] | H. Matsuoka and K.-I. Nakamura, A stable finite difference method for a Cahn-Hilliard type equation with long-range interaction, Sci. Rep. Kanazawa Univ. 57 (2013), 13-34. |
[281] | S. Mikhailov, M. Hildebrand and G. Ertl, Nonequilibrium nanostructures in condensed reactive systems, in Coherent Structures in Complex Systems (Sitges, 2000), Vol. 567,252-269,2001. |
[282] | R.M. Mininni, A. Miranville and S. Romanelli, Higher-order Cahn-Hilliard equations with dynamic boundary conditions, J. Math. Anal. Appl. 449 (2017), 1321-1339. |
[283] | S. Minjeaud, An unconditionally stable uncoupled scheme for a triphasic Cahn-Hilliard/NavierStokes model, Numer. Methods Partial Diff. Eqns. 29 (2013), 584-618. |
[284] | A. Miranville, Some generalizations of the Cahn-Hilliard equation, Asymptotic Anal. 22 (2000), 235-259. |
[285] | A. Miranville, Long-time behavior of some models of Cahn-Hilliard equations in deformable continua, Nonlinear Anal. Real World Appl. 2 (2001), 273-304. |
[286] | A. Miranville, Consistent models of Cahn-Hilliard-Gurtin equations with Neumann boundary conditions, Physica D 158 (2001), 233-257. |
[287] | A. Miranville, Asymptotic behavior of the Cahn-Hilliard-Oono equation, J. Appl. Anal. Comput. 1 (2011), 523-536. |
[288] | A. Miranville, Asymptotic behaviour of a generalized Cahn-Hilliard equation with a proliferation term, Appl. Anal. 92 (2013), 1308-1321. |
[289] | A. Miranville, Asymptotic behavior of a sixth-order Cahn-Hilliard system, Cent. Eur. J. Math. 12 (2014), 141-154. |
[290] | A. Miranville, Sixth-order Cahn-Hilliard equations with logarithmic nonlinear terms, Appl. Anal. 94 (2015), 2133-2146. |
[291] | A. Miranville, Sixth-order Cahn-Hilliard systems with dynamic boundary conditions, Math. Methods Appl. Sci. 38 (2015), 1127-1145. |
[292] | A. Miranville, A generalized Cahn-Hilliard equation with logarithmic potentials, Continuous and distributed systems Ⅱ, Stud. Systems Decis. Control, Springer, Vol. 30,137-148,2015. |
[293] | A. Miranville, On the phase-field-crystal model with logarithmic nonlinear terms, RACSAM 110 (2016), 145-157. |
[294] | A. Miranville and A. Piétrus, A new formulation of the Cahn-Hilliard equation, Nonlinear Anal. Real World Appl. 7 (2006), 285-307. |
[295] | A. Miranville and A. Rougirel, Local and asymptotic analysis of the flow generated by the CahnHilliard-Gurtin equations, Z. Angew. Math. Phys. 57 (2006), 244-268. |
[296] | A. Miranville, W. Saoud and R. Talhouk, Asymptotic behavior of a model for order-disorder and phase separation, Asymptot. Anal. 103 (2017), 57-76. |
[297] | A. Miranville and G. Schimperna, Nonisothermal phase separation based on a microforce balance, Discrete Contin. Dyn. Systems Ser. B 5 (2005), 753-768. |
[298] | A. Miranville and G. Schimperna, Generalized Cahn-Hilliard equations for multicomponent alloys, Adv. Math. Sci. Appl. 19 (2009), 131-154. |
[299] | A. Miranville and G. Schimperna, On a doubly nonlinear Cahn-Hilliard-Gurtin system, Discrete Contin. Dyn. Systems Ser. B 14 (2010), 675-697. |
[300] | A. Miranville and R. Temam, On the Cahn-Hilliard-Oono-Navier-Stokes equations with singular potentials, Appl. Anal. 95 (2016), 2609-2624. |
[301] | A. Miranville and S. Zelik, Robust exponential attractors for Cahn-Hilliard type equations with singular potentials, Math. Methods Appl. Sci. 27 (2004), 545-582. |
[302] | A. Miranville and S. Zelik, Exponential attractors for the Cahn-Hilliard equation with dynamic boundary conditions, Math. Methods Appl. Sci. 28 (2005), 709-735. |
[303] | A. Miranville and S. Zelik, Attractors for dissipative partial differential equations in bounded and unbounded domains, in Handbook of Differential Equations, Evolutionary Partial Differential Equations, Vol. 4, C. M. Dafermos and M. Pokorny eds. , Elsevier, Amsterdam, 103-200,2008. |
[304] | A. Miranville and S. Zelik, Doubly nonlinear Cahn-Hilliard-Gurtin equations, Hokkaido Math. J. 38 (2009), 315-360. |
[305] | A. Miranville and S. Zelik, The Cahn-Hilliard equation with singular potentials and dynamic boundary conditions, Discrete Contin. Dyn. Systems 28 (2010), 275-310. |
[306] | F. Nabet, Convergence of a finite-volume scheme for the Cahn-Hilliard equation with dynamic boundary conditions, IMA J. Numer. Anal. 36 (2016), 1898-1942. |
[307] | B. Nicolaenko and B. Scheurer, Low dimensional behaviour of the pattern formation equations, in Trends and practice of nonlinear analysis, V. Lakshmikantham ed. , North-Holland, 1985. |
[308] | B. Nicolaenko, B. Scheurer and R. Temam, Some global dynamical properties of a class of pattern formation equations, Commun. Partial Diff. Eqns. 14 (1989), 245-297. |
[309] | A. Novick-Cohen, Energy methods for the Cahn-Hilliard equation, Quart. Appl. Math. 46 (1988), 681-690. |
[310] | A. Novick-Cohen, On the viscous Cahn-Hilliard equation, in Material instabilities in continuum and related problems, J. M. Ball ed. , Oxford University Press, Oxford, 329-342,1988. |
[311] | A. Novick-Cohen, The Cahn-Hilliard equation: Mathematical and modeling perspectives, Adv. Math. Sci. Appl. 8 (1998), 965-985. |
[312] | A. Novick-Cohen, Triple-junction motion for an Allen-Cahn/Cahn-Hilliard system, Physica D 137 (2000), 1-24. |
[313] | A. Novick-Cohen, The Cahn-Hilliard equation, in Handbook of Differential Equations, Evolutionary Partial Differential Equations, Vol. 4, C. M. Dafermos and M. Pokorny eds. , Elsevier, Amsterdam, 201-228,2008. |
[314] | Y. Oono and S. Puri, Computationally efficient modeling of ordering of quenched phases, Phys. Rev. Lett. 58 (1987), 836-839. |
[315] | A. Oron, S.H. Davis and S.G. Bankoff, Long-scale evolution of thin liquid films, Rev. Mod. Phys. 69 (1997), 931-980. |
[316] | I. Pawłow and G. Schimperna, On a Cahn-Hilliard model with nonlinear diffusion, SIAM J. Math. Anal. 45 (2013), 31-63. |
[317] | I. Pawłow and G. Schimperna, A Cahn-Hilliard equation with singular diffusion, J. Diff. Eqns. 254 (2013), 779-803. |
[318] | I. Pawłow and W.M. Zajaczkowski, Strong solvability of 3-D Cahn-Hilliard system in elastic solids, Math. Methods Appl. Sci. 32 (2008), 879-914. |
[319] | I. Pawłow and W.M. Zajaczkowski, Weak solutions to 3-D Cahn-Hilliard system in elastic solids, Topol. Methods Nonlinear Anal. 32 (2008), 347-377. |
[320] | I. Pawłow and W.M. Zajaczkowski, Global regular solutions to Cahn-Hilliard system coupled with viscoelasticity, Math. Methods Appl. Sci. 32 (2009), 2197-2242. |
[321] | I. Pawłow and W.M. Zajaczkowski, Long time behaviour of a Cahn-Hilliard system coupled with viscoelasticity, Ann. Polon. Math. 98 (2010), 1-21. |
[322] | I. Pawłow and W. Zajaczkowski, A sixth order Cahn-Hilliard type equation arising in oil-watersurfactant mixtures, Commun. Pure Appl. Anal. 10 (2011), 1823-1847. |
[323] | I. Pawłow and W. Zajaczkowski, On a class of sixth order viscous Cahn-Hilliard type equations, Discrete Contin. Dyn. Systems Ser. S 6 (2013), 517-546. |
[324] | M. Pierre, Habilitation thesis, Universite de Poitiers, 2011. ´ |
[325] | P. Podio-Guidugli, Models of phase segregation and diffusion of atomic species on a lattice, Ric. Mat. 55 (2006), 105-118. |
[326] | J. Prüss, R. Racke and S. Zheng, Maximal regularity and asymptotic behavior of solutions for the Cahn-Hilliard equation with dynamic boundary conditions, Ann. Mat. Pura Appl. (4) 185 (2006), 627-648. |
[327] | J. Prüss, V. Vergara and R. Zacher, Well-posedness and long-time behaviour for the non-isothermal Cahn-Hilliard equation with memory, Discrete Contin. Dyn. Systems 26 (2010), 625-647. |
[328] | T. Qian, X.-P. Wang and P. Sheng, A variational approach to moving contact line hydrodynamics, J. Fluid Mech. 564 (2006), 333-360. |
[329] | R. Racke and S. Zheng, The Cahn-Hilliard equation with dynamic boundary conditions, Adv. Diff. Eqns. 8 (2003), 83-110. |
[330] | A. Rajagopal, P. Fischer, E. Kuhl and P. Steinmann, Natural element analysis of the Cahn-Hilliard phase-field model, Comput. Mech. 46 (2010), 471-493. |
[331] | A. Roggensack and C. Kraus, Existence of weak solutions for the Cahn-Hilliard reaction model including elastic effects and damage, J. Partial Diff. Eqns. 30 (2017), 111-145. |
[332] | R. Rossi, On two classes of generalized viscous Cahn-Hilliard equations, Commun. Pure Appl. Anal. 4 (2005), 405-430. |
[333] | R. Rossi, Global attractor for the weak solutions of a class of viscous Cahn-Hilliard equations, in Dissipative phase transitions, Ser. Adv. Math. Appl. Sci. , Vol. 71, World Sci. Publ. , Hackensack, NJ, 247-268,2006. |
[334] | A. Rougirel, Convergence to steady state and attractors for doubly nonlinear equations, J. Math. Anal. Appl. 339 (2008), 281-294. |
[335] | P. Rybka and K.-H. Hoffmann, Convergence of solutions to Cahn-Hilliard equation, Commun. Partial Diff. Eqns. 24 (1999), 1055-1077. |
[336] | A. Sariaydin-Filibelioglu, B. Karaszen and M. Uzunca, Energy stable interior penalty discontinuous Galerkin finite element method for Cahn-Hilliard equation, Int. J. Nonlinear Sci. Numer. Simul. 18 (2017), 303-314. |
[337] | G. Savaré and A. Visintin, Variational convergence of nonlinear diffusion equations: applications to concentrated capacity problems with change of phase, Atti Accad. Naz. Lincei Cl. Sci. Fis. Mat. Natur. Rend. Lincei (9) Mat. Appl. 8 (1997), 49-89. |
[338] | A. Savostianov and S. Zelik, Global well-posedness and attractors for the hyperbolic CahnHilliard-Oono equation in the whole space, Math. Models Methods Appl. Sci. 26 (2016), 1357-1384. |
[339] | A. Savostianov and S. Zelik, Finite dimensionality of the attractor for the hyperbolic CahnHilliard-Oono equation in R3, Math. Methods Appl. Sci. 39 (2016), 1254-1267. |
[340] | R. Scala and G. Schimperna, On the viscous Cahn-Hilliard equation with singular potential and inertial term, AIMS Math. 1 (2016), 64-76. |
[341] | G. Schimperna, Weak solution to a phase-field transmission problem in a concentrated capacity, Math. Methods Appl. Sci. 22 (1999), 1235-1254. |
[342] | G. Schimperna, Global attractor for Cahn-Hilliard equations with nonconstant mobility, Nonlinearity 20 (2007), 2365-2387. |
[343] | G. Schimperna and S. Zelik, Existence of solutions and separation from singularities for a class of fourth order degenerate parabolic equations, Trans. Amer. Math. Soc. 365 (2013), 3799-3829. |
[344] | J. Shen and X. Yang, Numerical approximations of Allen-Cahn and Cahn-Hilliard equations, Discrete Contin. Dyn. Systems 28 (2010), 1669-1691. |
[345] | J. Shen and X. Yang, Energy stable schemes for Cahn-Hilliard phase-field model of two-phase incompressible flows, Chinese Ann. Math., Ser. B 31 (2010), 743-758. |
[346] | W. Shen and S. Zheng, On the coupled Cahn-Hilliard equations, Commun. Partial Diff. Eqns. 18 (1993), 701-727. |
[347] | R.H. Stogner, G.F. Carey and B.T. Murray, Approximation of Cahn-Hilliard diffuse interface models using parallel adaptative mesh refinement and coarsening with C1 elements, Int. J. Numer. Methods Engrg. 76 (2008), 636-661. |
[348] | J.E. Taylor, Mean curvature and weighted mean curvature, Acta Metall. Mater. 40 (1992), 1475-1495. |
[349] | R. Temam, Infinite-dimensional dynamical systems in mechanics and physics, Second edition, Applied Mathematical Sciences, Vol. 68, Springer-Verlag, New York, 1997. |
[350] | U. Thiele and E. Knobloch, Thin liquid films on a slightly inclined heated plate, Physica D 190 (2004), 213-248. |
[351] | G. Tierra and F. Guillén-González, Numerical methods for solving the Cahn-Hilliard equation and its applicability to related energy-based models, Arch. Comput. Methods Engrg. 22 (2015), 269-289. |
[352] | S. Torabi, J. Lowengrub, A. Voigt and S. Wise, A new phase-field model for strongly anisotropic systems, Proc. R. Soc. A 465 (2009), 1337-1359. |
[353] | S. Tremaine, On the origin of irregular structure in Saturn's rings, Astron. J. 125 (2003), 894-901. |
[354] | J. Verdasca, P. Borckmans and G. Dewel, Chemically frozen phase separation in an adsorbed layer, Phys. Review E 52 (1995), 4616-4619. |
[355] | S. Villain-Guillot, Phases modulées et dynamique de Cahn-Hilliard, Habilitation thesis, Université Bordeaux I, 2010. |
[356] | C. Wang and S.M. Wise, Global smooth solutions of the modified phase field crystal equation, Methods Appl. Anal. 17 (2010), 191-212. |
[357] | C. Wang and S.M. Wise, An energy stable and convergent finite difference scheme for the modified phase field crystal equation, SIAM J. Numer. Anal. 49 (2011), 945-969. |
[358] | W. Wang, L. Chen and J. Zhou, Postprocessing mixed finite element methods for solving CahnHilliard equation: methods and error analysis, J. Sci. Comput. 67 (2016), 724-746. |
[359] | X. Wang and H. Wu, Long-time behavior for the Hele-Shaw-Cahn-Hilliard system, Asymptot. Anal. 78 (2012), 217-245. |
[360] | X. Wang and Z. Zhang, Well-posedness of the Hele-Shaw-Cahn-Hilliard system, Ann. Inst. H. Poincare Anal. Non Linéaire 30 (2013), 367-384. |
[361] | S.J. Watson, F. Otto, B. Rubinstein and S.H. Davis, Coarsening dynamics of the convective CahnHilliard equation, Physica D 178 (2003), 127-148. |
[362] | G.N. Wells, E. Kuhl and K. Garikipati, A discontinuous Galerkin method for Cahn-Hilliard equation, J. Comput. Phys. 218 (2006), 860-877. |
[363] | A.A. Wheeler and G.B. McFadden, On the notion of ξ-vector and stress tensor for a general class of anisotropic diffuse interface models, Proc. R. Soc. London Ser. A 453 (1997), 1611-1630. |
[364] | M. Wilke, Lp-theory for a Cahn-Hilliard-Gurtin system, Evol. Eqns. Control Theory 1 (2012), 393-429. |
[365] | S.M. Wise, Unconditionally stable finite difference, nonlinear multigrid simulations of the CahnHilliard-Hele-Shaw system of equations, J. Sci. Comput. 44 (2010), 38-68. |
[366] | S. Wise, J. Kim and J. Lowengrub, Solving the regularized, strongly anisotropic Cahn-Hilliard equation by an adaptive nonlinear multigrid method, J. Comput. Phys. 226 (2007), 414-446. |
[367] | S.M. Wise, C. Wang and J.S. Lowengrub, An energy stable and convergent finite difference scheme for the phase field crystal equation, SIAM J. Numer. Anal. 47 (2009), 2269-2288. |
[368] | H. Wu and S. Zheng, Convergence to equilibrium for the Cahn-Hilliard equation with dynamic boundary conditions, J. Diff. Eqns. 204 (2004), 511-531. |
[369] | Y. Xia, Y. Xu and C.-W. Shu, Application of the local discontinuous Galerkin method for the Allen-Cahn/Cahn-Hilliard system, Commun. Comput. Phys. 5 (2009), 821-835. |
[370] | J. Yin and C. Liu, Cahn-Hilliard type equations with concentration dependent mobility, in Mathematical methods and models in phase transitions, A. Miranville ed. , Nova Sci. Publ. , New York, 79-93,2005. |
[371] | B. You and F. Li, Well-posedness and global attractor of the Cahn-Hilliard-Brinkman system with dynamic boundary conditions, Dyn. Partial Diff. Eqns. 13 (2016), 75-90. |
[372] | P. Yue, J.J. Feng, C. Liu and J. Shen, A diffuse-interface method for simulating two-phase flows of complex fluids, J. Fluid Mech. 515 (2004), 293-317. |
[373] | T. Zhang and Q. Wang, Cahn-Hilliard vs singular Cahn-Hilliard equations in phase field modeling, Commun. Comput. Phys. 7 (2010), 362-382. |
[374] | X. Zhang and C. Liu, Existence of solutions to the Cahn-Hilliard/Allen-Cahn equation with degenerate mobility, Electron. J. Diff. Eqns. 2016 (2016), 1-22. |
[375] | L.-Y. Zhao, H. Wu and H.-Y. Huang, Convergence to equilibrium for a phase-field model for the mixture of two incompressible fluids, Commun. Math. Sci. 7 (2009), 939-962. |
[376] | S. Zheng, Asymptotic behavior of solution to the Cahn-Hilliard equation, Appl. Anal. 23 (1986), 165-184. |
[377] | X. Zheng, C. Yang, X.-C. Cai and D. Keyes, A parallel domain decomposition-based implicit method for the Cahn-Hilliard-Cook phase-field equation in 3D, J. Comput. Phys. 285 (2015), 55-70. |
[378] | J.X. Zhou and M.E. Li, Solving phase field equations with a meshless method, Commun. Numer. Methods Engrg. 22 (2006), 1109-1115. |
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32. | Kazuki Shimura, Shuji Yoshikawa, A new conservative finite difference scheme for 1D Cahn–Hilliard equation coupled with elasticity, 2022, 28, 1425-6908, 311, 10.1515/jaa-2021-2071 | |
33. | Pierluigi Colli, Takeshi Fukao, Luca Scarpa, A Cahn–Hilliard system with forward-backward dynamic boundary condition and non-smooth potentials, 2022, 22, 1424-3199, 10.1007/s00028-022-00847-x | |
34. | Federica Bubba, Alexandre Poulain, A nonnegativity preserving scheme for the relaxed Cahn–Hilliard equation with single-well potential and degenerate mobility, 2022, 56, 2822-7840, 1741, 10.1051/m2an/2022050 | |
35. | Tomasz Dlotko, Navier–Stokes–Cahn–Hilliard system of equations, 2022, 63, 0022-2488, 111511, 10.1063/5.0097137 | |
36. | Revanth Mattey, Susanta Ghosh, A novel sequential method to train physics informed neural networks for Allen Cahn and Cahn Hilliard equations, 2022, 390, 00457825, 114474, 10.1016/j.cma.2021.114474 | |
37. | Azer Khanmamedov, Attractors for some models of the Cahn–Hilliard equation with the inertial term, 2023, 36, 0951-7715, 1120, 10.1088/1361-6544/acad5d | |
38. | Kei Fong Lam, Global and exponential attractors for a Cahn–Hilliard equation with logarithmic potentials and mass source, 2022, 312, 00220396, 237, 10.1016/j.jde.2021.12.014 | |
39. | Akihiro Umeda, Yuta Wakasugi, Shuji Yoshikawa, Energy-conserving finite difference schemes for nonlinear wave equations with dynamic boundary conditions, 2022, 171, 01689274, 1, 10.1016/j.apnum.2021.08.009 | |
40. | Nitu Lakhmara, Hari Shankar Mahato, Homogenization of a coupled incompressible Stokes–Cahn–Hilliard system modeling binary fluid mixture in a porous medium, 2022, 222, 0362546X, 112927, 10.1016/j.na.2022.112927 | |
41. | Paula Harder, Balázs Kovács, Error estimates for the Cahn–Hilliard equation with dynamic boundary conditions, 2022, 42, 0272-4979, 2589, 10.1093/imanum/drab045 | |
42. | Cedric Aaron Beschle, Balázs Kovács, Stability and error estimates for non-linear Cahn–Hilliard-type equations on evolving surfaces, 2022, 151, 0029-599X, 1, 10.1007/s00211-022-01280-5 | |
43. | Wu Jihui, Wang Shu, On the degenerate Cahn–Hilliard equation: Global existence and entropy estimates of weak solutions, 2020, 119, 18758576, 1, 10.3233/ASY-191563 | |
44. | Anna Song, Generation of Tubular and Membranous Shape Textures with Curvature Functionals, 2022, 64, 0924-9907, 17, 10.1007/s10851-021-01049-9 | |
45. | Emmanuel Y. Medina, Elson M. Toledo, Iury Igreja, Bernardo M. Rocha, A stabilized hybrid discontinuous Galerkin method for the Cahn–Hilliard equation, 2022, 406, 03770427, 114025, 10.1016/j.cam.2021.114025 | |
46. | Jürgen Geiser, Lutz Schimansky-Geier, 2022, 2425, 0094-243X, 420006, 10.1063/5.0081363 | |
47. | Matthieu Brachet, Philippe Parnaudeau, Morgan Pierre, Convergence to equilibrium for time and space discretizations of the Cahn-Hilliard equation, 2022, 15, 1937-1632, 1987, 10.3934/dcdss.2022110 | |
48. | Olena Burkovska, Max Gunzburger, On a nonlocal Cahn–Hilliard model permitting sharp interfaces, 2021, 31, 0218-2025, 1749, 10.1142/S021820252150038X | |
49. | Elisabetta Rocca, Giulio Schimperna, Andrea Signori, On a Cahn–Hilliard–Keller–Segel model with generalized logistic source describing tumor growth, 2023, 343, 00220396, 530, 10.1016/j.jde.2022.10.026 | |
50. | Pierluigi Colli, Takeshi Fukao, Luca Scarpa, The Cahn--Hilliard Equation with Forward-Backward Dynamic Boundary Condition via Vanishing Viscosity, 2022, 54, 0036-1410, 3292, 10.1137/21M142441X | |
51. | Daniel Acosta-Soba, Francisco Guillén-González, J. Rafael Rodríguez-Galván, An upwind DG scheme preserving the maximum principle for the convective Cahn-Hilliard model, 2023, 92, 1017-1398, 1589, 10.1007/s11075-022-01355-2 | |
52. | A. N. Kulikov, D. A. Kulikov, Local Bifurcations of Invariant Manifolds of the Cahn–Hilliard–Oono Equation, 2023, 44, 1995-0802, 1003, 10.1134/S1995080223030174 | |
53. | José M. Mazón, Julián Toledo, Cahn–Hilliard equations on random walk spaces, 2023, 21, 0219-5305, 959, 10.1142/S0219530523500045 | |
54. | Zehra Şen, Azer Khanmamedov, The Cahn-Hilliard/Allen-Cahn equation with inertial and proliferation terms, 2024, 530, 0022247X, 127736, 10.1016/j.jmaa.2023.127736 | |
55. | Chaeyoung Lee, Sangkwon Kim, Soobin Kwak, Youngjin Hwang, Seokjun Ham, Seungyoon Kang, Junseok Kim, Semi-automatic fingerprint image restoration algorithm using a partial differential equation, 2023, 8, 2473-6988, 27528, 10.3934/math.20231408 | |
56. | Mariano Torrisi, Rita Tracinà, Symmetries and Conservation Laws for a Class of Fourth-Order Reaction–Diffusion–Advection Equations, 2023, 15, 2073-8994, 1936, 10.3390/sym15101936 | |
57. | Vincent Giovangigli, Yoann Le Calvez, Flore Nabet, Symmetrization and Local Existence of Strong Solutions for Diffuse Interface Fluid Models, 2023, 25, 1422-6928, 10.1007/s00021-023-00825-4 | |
58. | Hussein Fakih, Mahdi Faour, Wafa Saoud, Yahia Awad, On the complex version of the Cahn–Hilliard–Oono type equation for long interactions phase separation, 2024, 0, 2956-7068, 10.2478/ijmce-2024-0018 | |
59. | Parisa Khodabakhshi, Olena Burkovska, Karen Willcox, Max Gunzburger, Multifidelity methods for uncertainty quantification of a nonlocal model for phase changes in materials, 2024, 297, 00457949, 107328, 10.1016/j.compstruc.2024.107328 | |
60. | P. Suman Prakash, P. Kiran Rao, E. Suresh Babu, Surbhi Bhatia Khan, Ahlam Almusharraf, Mohammad Tabrez Quasim, Decoupled SculptorGAN Framework for 3D Reconstruction and Enhanced Segmentation of Kidney Tumors in CT Images, 2024, 12, 2169-3536, 62189, 10.1109/ACCESS.2024.3389504 | |
61. | Hussein Fakih, Marwa Badreddine, Hawraa Alsayed, Yahia Awad, On a generalization of the Cahn-Hilliard type equation with logarithmic nonlinearities for formation of islands, 2024, 0, 2956-7068, 10.2478/ijmce-2025-0008 | |
62. | Saulo Orizaga, Thomas Witelski, IMEX methods for thin-film equations and Cahn–Hilliard equations with variable mobility, 2024, 243, 09270256, 113145, 10.1016/j.commatsci.2024.113145 | |
63. | Andrea Cavagna, Javier Cristín, Irene Giardina, Mario Veca, From noise on the sites to noise on the links: Discretizing the conserved Kardar-Parisi-Zhang equation in real space, 2024, 109, 2470-0045, 10.1103/PhysRevE.109.064136 | |
64. | Saulo Orizaga, Ogochukwu Ifeacho, Sampson Owusu, On an efficient numerical procedure for the Functionalized Cahn-Hilliard equation, 2024, 9, 2473-6988, 20773, 10.3934/math.20241010 | |
65. | Elisa Davoli, Chiara Gavioli, Luca Lombardini, Existence results for Cahn–Hilliard-type systems driven by nonlocal integrodifferential operators with singular kernels, 2024, 248, 0362546X, 113623, 10.1016/j.na.2024.113623 | |
66. | Saulo Orizaga, Gilberto González-Parra, Logan Forman, Jesus Villegas-Villanueva, Solving Allen-Cahn equations with periodic and nonperiodic boundary conditions using mimetic finite-difference operators, 2025, 484, 00963003, 128993, 10.1016/j.amc.2024.128993 | |
67. | Dieunel Dor, Morgan Pierre, A robust family of exponential attractors for a linear time discretization of the Cahn-Hilliard equation with a source term, 2024, 58, 2822-7840, 1755, 10.1051/m2an/2024061 | |
68. | Darko Mitrovic, Andrej Novak, Navigating the Complex Landscape of Shock Filter Cahn–Hilliard Equation: From Regularized to Entropy Solutions, 2024, 248, 0003-9527, 10.1007/s00205-024-02057-w | |
69. | Chang Li, Fanhong Kong, Lei Feng, Han Sun, Xing Han, Fenghua Luo, Research on Ni-WC Coating and a Carbide Solidification Simulation Mechanism of PTAW on the Descaling Roll Surface, 2024, 14, 2079-6412, 1490, 10.3390/coatings14121490 | |
70. | A. N. Kulikov, D. A. Kulikov, Convective Cahn–Hilliard–Oono Equation, 2024, 64, 0965-5425, 2399, 10.1134/S0965542524701343 | |
71. | Nitu Lakhmara, Hari Shankar Mahato, Analysis of a Cahn–Hilliard model for a three-phase flow problem, 2025, 150, 0022-0833, 10.1007/s10665-024-10418-3 | |
72. | Qingyu Li, Juanjuan Qiao, Guichao Wang, Songying Chen, The Taylor flow characteristic and mass transfer in curved T-microchannels, 2025, 37, 1070-6631, 10.1063/5.0252466 | |
73. | P. Mchedlov-Petrosyan, L. Davydov, Cahn-Hilliard model with Schlögl Reactions: interplay of equilibrium and non-equilibrium phase transitions. II. Memory effects, 2025, 28, 2224-9079, 13601, 10.5488/cmp.28.13601 |