Analysis of drain induced barrier lowering for junctionless double gate MOSFET using ferroelectric negative capacitance effect

Introduction

In this paper we study an atomistic model for (possibly heterogeneous) nanowires. We consider a scaling of the energy that corresponds to a reduction of the system from $N$ dimensions to one dimension and, in addition, accounts for transitions between different equilibria.

Specifically, in the homogeneous case, we study the asymptotic behaviour of the energy defined by

where $p>1$ and $u$ is a deformation of the portion of the lattice $\varepsilon \mathbb{Z}^N$ modelling the nanowire; the small parameter $\varepsilon >0$ represents the atomic distance and $R>0$ is sufficiently large to include a certain number of interactions beyond nearest neighbours. The above sum is taken over a "thin" domain, i.e., a domain consisting of a few lines of atoms (for the precise formula see (1.4)); as the lattice distance converges to zero, we perform a discrete to continuum limit and a dimension reduction simultaneously.

This model was first studied in [14,15] under the assumption that the admissible deformations satisfy the non-interpenetration condition, namely, that the Jacobian determinant of a suitably defined piecewise affine interpolation of $u$ is positive. Here we remove such assumption and we show that, by incorporating into the energy the effect of interactions in a certain finite range, one can recover the results of [14,15] and get even further insight into the problem. More precisely, we obtain an effective energy that accounts for the effects of changes of orientation in the lattice. The latter are thus allowed, but energetically penalised. We remark that, in dimension two, our analysis corresponds to the first-order $\Gamma$-limit of a functional of the kind studied in [1,18] without non-interpenetration assumptions. We also point out that the effects of long range interactions in non-convex lattice systems have already been analysed in [7,5,6] in the one-dimensional case.

For the scaling of (0.1), we obtain a complete description of the $\Gamma$-limit with respect to two different topologies (Theorems 5.1 and 5.4). It turns out that the $\Gamma$-limit with respect to the topology used in [14,15] is trivial (see Remark 4), that is, one can exhibit recovery sequences for which the gradient always lies in the same energy well up to an asymptotically vanishing correction. In order to see the effects of changes of orientation in the nanowire, we introduce a stronger topology which is sensitive to them. In this case, for each change of orientation, the $\Gamma$-limit gives a finite positive contribution which is characterised by a discrete optimal transition problem. Moreover, one can prove that if we prescribe affine boundary conditions of the type $x\mapsto Bx$ with $\text{dist}(B;SO(N))$ sufficiently small, then recovery sequences for minimisers will always preserve orientation (Remark 6). In this respect our model is consistent with the non-interpenetration condition. On the other hand, we also show that minimisers may violate such condition if we add to the functionals pathological loading terms which force the deformations to overcome the energetic barrier between equilibria with opposite orientation (see Section 6 and Remark 7).

The $\Gamma$-limit is nontrivial, also in the weaker topology, when one considers heterogeneous nanowires, which consist of components with different equilibria, arranged longitudinally; i.e., the interface between the components is a cross-section of the rod. In this case, we prove an estimate on the minimal energy spent to match the equilibria. Precisely, denoting by $k\in\mathbb{N}$ the number of atomic layers of the nanowire, we show that the minimal cost grows faster than $k^{N-1}$. The proof of such result (Theorem 2.2) follows as an application of [2,Theorem 3.1]. Such lower bound is to be compared with the estimate that one can prove in the case of a two-or three-dimensional model accounting for dislocations. This is discussed in Section 7 where we compare the minimal energy of heterogeneous defect-free systems and the minimal energy of heterogeneous systems containing dislocations. It turns out that for sufficiently large values of $k$, the latter are energetically preferred since their energy may grow exactly like $k^{N-1}$ (see Remark 8). In this respect our result is consistent with the one proven in [14,15] under the non-interpenetration assumption. We recall that the first variational justification of dislocation nucleation in nanowire heterostructures was obtained in [17] in the context of non-linear elasticity. This result was later generalised to a discrete to continuum setting in [14,15] under the non-interpenetration condition, and is here validated without the latter assumption. More recently, variational models for misfit dislocations at semi-coherent interfaces and in elastic thin films have been proposed in [10] and [11] respectively.

The paper is organised as follows. In Section 1 we introduce the model. In Section 1 we introduce the minimal costs to bridge different equilibria and study their dependence on the thickness of the nanowire. In Sections 3-5, performing a discrete to continuum limit and a dimension reduction simultaneously, we characterise the $\Gamma$-limit of the energy functional for different choices of the topology (Theorems 5.1 and 5.4). All the results are stated in the general case of heterogeneous nanowires. In Section 6 we discuss the effect of boundary conditions on the $\Gamma$-limit and briefly study a model including external forces (only in the homogeneous case, for simplicity). In the final part of the paper, Section 7, we compare the model for defect-free nanowires with models including dislocations at the interface, showing that the latter are energetically favoured.

Notation. We recall some basic notions of geometric measure theory for which we refer to [3]. Given a bounded open set $\Omega \subset\mathbb{R}^N$, $N\ge 2$, and $M\ge1$, $BV(\Omega ;\mathbb{R}^M)$ denotes the space of functions of bounded variation; i.e., of functions $u\in L^{1}(\Omega ;\mathbb{R}^M)$ whose distributional gradient $\mathrm{D} u$ is a Radon measure on $\Omega$ with $|\mathrm{D} u|(\Omega ) < +\infty$, where $|\mathrm{D} u|$ is the total variation of $\mathrm{D} u$. If $u\in BV(\Omega ;\mathbb{R}^M)$, the symbol $\nabla u$ stands for the density of the absolutely continuous part of $\mathrm{D} u$ with respect to the $N$-dimensional Lebesgue measure $\mathcal{L}^N$. We denote by $J_u$ the jump set of $u$, by $u^+$ and $u^-$ the traces of $u$ on $J_u$, and by $\nu_u(x)$ the measure theoretic inner normal to $J_u$ at $x$, which is defined for $\mathcal{H}^{N{-} 1}$-a.e. $x \in J_u$, where $\mathcal{H}^{N{-}1}$ is the $(N{-}1)$-dimensional Hausdorff measure. A function $u\in BV(\Omega ;\mathbb{R}^M)$ is said to be a special function of bounded variation if $\mathrm{D} u - \nabla u \, \mathcal{L}^N$ is concentrated on $J_u$; in this case one writes $u\in SBV(\Omega ;\mathbb{R}^M)$. Given a set $E\subset \Omega$, we denote by $P(E, \Omega )$ its relative perimeter in $\Omega$ and by $\partial^*E$ its reduced boundary. We recall that a partition $\{E_i\}_{i\in\mathbb{N}}$ of $\Omega$ is called a Caccioppoli partition if $\sum_{i\in\mathbb{N}} P(E_i, \Omega ) < +\infty$. Given a rectifiable set $K\subset\Omega$, we say that a Caccioppoli partition $\{E_i\}_{i\in\mathbb{N}}$ of $\Omega$ is subordinated to $K$ if for every $i\in\mathbb{N}$ the reduced boundary $\partial^* E_i$ of $E_i$ is contained in $K$, up to a $\mathcal{H}^{N-1}$-negligible set.

For $N\ge2$, ${{\mathbb{M}}^{N\times N}}$ is the set of real $N{\times} N$ matrices, $GL^+(N)$ is the set of matrices with positive determinant, $O(N)$ is the set of orthogonal matrices, and $SO(N)$ is the set of rotations. We denote by $I$ the identity matrix and $J$ the reflection matrix such that $Je_1 = -e_1$ and $Je_i = e_i$ for $i = 2, \dots, N$, where $\{e_i\colon i = 2, \dots, N\}$ is the canonical basis in $\mathbb{R}^N$. The symbol $\text{co}(X)$ stands for the convex hull of a set $X$ in ${{\mathbb{M}}^{N\times N}}$. Moreover, given $N{+}1$ points $x_0, x_1, \dots, x_N\in\mathbb{R}^N$, we denote by $[x_0, x_1, \dots, x_N]$ the simplex determined by all convex combinations of those points.

Finally, $\mathcal{U}$ is the class of subsets of $(-L, L)$ that are disjoint union of a finite number of open intervals.

In the paper, the same letter $C$ denotes various positive constants whose precise value may change from place to place.

1.   Setting of the problem

We study the dimension reduction of a discrete model for heterogeneous nanowires. Let $L>0$, $k\in \mathbb{N}$, $\Omega _{k\varepsilon } : = (-L, L)\times (-k\varepsilon, k\varepsilon )^{N-1}$. Up to an affine deformation $H\in GL^+(N)$, we can reduce to the case where the lattice is $\mathbb{Z}^N$. Thus we consider the discrete thin domain $\mathcal{L}_\varepsilon(k) \subset \mathbb{R}^N$ defined as

where $\overline\Omega _{k\varepsilon}$ is the union of all hypercubes with vertices in $\varepsilon\mathbb{Z}^N$ that have non-empty intersection with $\Omega _{k\varepsilon}$. In the physically relevant case of $N = 3$, the set $\mathcal{L}_\varepsilon(k)$ models the crystal structure of a nanowire of length $2L$ and thickness $2k \varepsilon$, where $k$ is the number of parallel atomic planes. We will nonetheless state all the results for a general $N$, since their proof does not depend on the dimension. Notice that in definition (1.1) the dependence on $k$ is explicit; this parameter will indeed play a major role in the subsequent analysis.

The bonds between the atoms are defined by means of the so-called Kuhn decomposition, which is relevant for modelling some specific Bravais lattices. (See [2,Remark 2.6] for details on the treatment of some lattices in dimension two and three, such as the hexagonal or equilateral triangular, the face-centred cubic, and the body-centred cubic.) First we define a partition $\mathcal{T}_0$ of the unit cube $(0, 1)^N$ into $N$-simplices: we say that $T\in\mathcal{T}_0$ if the $(N{+}1)$-tuple of its vertices belongs to the set

where $S_N$ is the set of permutations of $N$ elements; see Figure 1. Next, we define $\mathcal{T}$ as the periodic extension of $\mathcal{T}_0$ to all of $\mathbb{R}^N$. We say that two nodes $x, y\in \mathbb{Z}^N$ are contiguous if there exists a simplex $T\in\mathcal{T}$ that has both $x$ and $y$ as its vertices. We set

If both simplices $[x_0, x_1, \dots, x_N]$ and $[y_0, x_1, \dots, x_N]$ belong to $\mathcal{T}$, then we say that $[x_0, x_1, \dots, x_N]$ and $[y_0, x_1, \dots, x_N]$ are neighbouring simplices (i.e., they share a facet) and $x_0$ and $y_0$ are opposite vertices. We set

and remark that, by periodicity, $B_1$ and $B_2$ do not depend on $x$.

We assume that $\mathcal{L}_\varepsilon(k)$ is composed of two species of atoms, occupying the points contained in the subsets

respectively, where $x = (x_1, \dots, x_N)$. The two species of atoms are characterised by equilibrium distances given by $\varepsilon$ and $\lambda\varepsilon$, respectively, where $\lambda\in(0, 1]$ is fixed; the case $\lambda\in(0, 1)$ models a heterogeneous nanowire, while the case $\lambda = 1$ refers to a homogeneous nanowire. Specifically, the total interaction energy relative to a deformation $u \colon\mathcal{L}_\varepsilon(k)\to\mathbb{R}^N$ is defined as

where $p>1$, $H\in GL^+(N)$, and the coefficient $c(\xi)$ is equal to some $c_1>0$ for $\xi\in B_1$ and to $c_2>0$ for $\xi\in B_2$.

To simplify the presentation, we restrict our attention to the case of $p$-harmonic potentials, though our analysis applies, without any significant change, to more general potentials satisfying polynomial growth conditions. More precisely, we may replace $\varepsilon _{\varepsilon }^{1, \lambda }(u, k)$ with

where $\phi\colon\mathbb{Z}^N\times\mathbb{R}\to [0, +\infty)$ is a positive potential such that

for some positive constants $C_1, C_2$. One could consider the case of potentials depending also on $x$ and satisfying suitable periodicity assumptions: this would require a more delicate analysis and would lead to a more complex formula for the $\Gamma$-limit.

In principle, all the results that we present in the sequel extend to the case when the two components of the nanowire have equilibria of the form $H^-$ and $H^+$, where $H^-, H^+\in GL^+(N)$. We have chosen to analyse the case when $H^+ = \lambda H^-$, since this is particularly meaningful in applications where one has misfit between two crystalline materials with the same lattice structure but different lattice distance at equilibrium (see e.g. [9,13]).

We study the limit behaviour of $\varepsilon _{\varepsilon }^{1, \lambda }(\cdot, k)$ as $\varepsilon\to 0^+$, thus performing simultaneously a discrete to continuum limit and a dimension reduction to a one-dimensional system. The limit functional was derived in [14,15] by means of $\Gamma$-convergence, under the assumption that the admissible deformations fulfil the non-interpenetration condition, namely, that the Jacobian determinant of (the piecewise affine interpolation of) any deformation is strictly positive almost everywhere. The non-interpenetration assumption was used in several parts of the analysis; in particular, it was needed to prove that the limit functional (dependent on $k$) scales like $k^N$ as $k\to\infty$.

The main novelty of the present paper is that we remove the non-interpenetration assumption made in [14,15], allowing for changes of orientations. Furthermore, in the study of the $\Gamma$-limit we define a stronger topology that accounts for such changes. In the proof of the new results, only those parts that differ from [14,15] will be shown in details.

In the sequel of the paper we will often consider the rescaled domain $\frac{1}{\varepsilon}\Omega _{k}\varepsilon$, which converges, as $\varepsilon\to0^+$, to the unbounded strip

We define the associated lattice and subsets

where $\overline\Omega _{k, \infty}$ is the union of all hypercubes with vertices in $\mathbb{Z}^N$ that have non-empty intersection with $\Omega _{k, \infty}$. For $u\colon \mathcal{L}_{\infty}(k) \to \mathbb{R}^N$ we define

We identify every deformation $u$ of the lattice $\mathcal{L}_{\varepsilon}(k)$ by its piecewise affine interpolation with respect to the triangulation $\varepsilon\mathcal{T}$. By a slight abuse of notation, such extension is still denoted by $u$. We can then define the domain of the functional (1.4) as

Similarly, for (1.5) we define

As customary in dimension reduction problems, we rescale the domain $\Omega _k\varepsilon$ to a fixed domain $\Omega _k$, independent of $\varepsilon$, by introducing the change of variables $z(x): = (x_1, \varepsilon x_2, \dots, \varepsilon x_N)$. Accordingly, for each $u\in\mathcal{A}_{\varepsilon}(\Omega _k\varepsilon )$ we define ${\tilde{u}} (x): = u(z(x))$. Moreover we set $\Omega _{k}: = A_\varepsilon^{-1}(\Omega _k\varepsilon ) = (-L, L)\times (-k, k)^{N-1}$, where $A_\varepsilon\in{{\mathbb{M}}^{N\times N}}$ is the diagonal matrix

i.e., $z(x) = A_\varepsilon x$. In this way we can recast the functionals (1.4) defined over varying domains into functionals defined on deformations of the fixed domain $\Omega _k$. Precisely we set

with

For later use it will be convenient to set the following notation:

2.   Definition and properties of minimal energies

We recall that, throughout the paper, $I$ is the identity matrix and $J$ is the reflection matrix such that $Je_1 = -e_1$ and $Je_i = e_i$ for $i = 2, \dots, N$.

We will study the $\Gamma$-limit of the sequence $\mathcal{I}_{\varepsilon }^{1, \lambda }(\cdot, k)$ as $\varepsilon\to 0^+$ for every fixed $k$. For this purpose we introduce the quantity $\gamma(P_1, P_2;k)$ for $P_1, P_2\in O(N)\cup \lambda\, O(N)$, which represents the minimum cost of a transition from a well to another. Specifically, for each $P_1 \in O(N)$ and $P_2\in \lambda\, O(N)$ we define

for $P_1, P_2 \in O(N)$

where

for $P_1, P_2 \in \lambda\, O(N)$

where

The next proposition shows that the relevant quantities defined through (2.1) are in fact four: the minimal costs of the transition at the interface between the energy wells $O(N)$ and $\lambda\, O(N)$ are provided in (2.2b) and (2.2c); the minimal cost of the transition between $SO(N)$ and $O(N){\setminus}SO(N)$ is provided in (2.2d); the one of the transition between $\lambda\, SO(N)$ and $\lambda\, O(N){\setminus}SO(N)$ is given in (2.2e). Moreover, the constants in (2.2d) and in (2.2e) are related by the proportionality rule (2.3).

Proposition 1. For each $k\in\mathbb{N}$, the function $\gamma$ satisfies for every $R, R'\in SO(N)$ and $Q, Q'\in O(N){\setminus}SO(N)$

Moreover,

Proof. First one notices that $\gamma(P_1, P_2;k) = \gamma(JP_1, JP_2;k)$. Hence, the proof of (2.2) relies on the construction of low energy transitions between two given rotations or two given rotoreflections, see [14,Proposition 2.4]. Finally, standard comparison arguments yield (2.3).

We now prove estimates on the asymptotic behaviour of $\gamma (I, \lambda I)$ and $\gamma (I, \lambda J)$ as $k\to \infty$, which have interesting consequences towards the comparison of this model with those accounting for dislocations in nanowires, see Section 7 below. Indeed, in Theorem 2.2 below we show that for $\lambda\neq1$ (heterogeneous nanowire) these constants grow faster than $k^{N-1}$, while it is known that the corresponding minimum cost for nanowires with dislocations scales like $k^{N-1}$ (see discussion at the end of Section 7). In contrast, we remark that for $\lambda = 1$ one has $\gamma (I, I) = 0$ and $\gamma (I, J)\simeq C k^{N-1}$. An essential tool in the proof of Theorem 2.2 is the following result.

Theorem 2.1.[2,Theorem 3.1] Let $u_\varepsilon\in\mathcal{A}_\varepsilon ((0, 1)^N)$ be a sequence such that

Then there are a subsequence (not relabelled) and a function $u\in W^{1, \infty}((0, 1)^N;\mathbb{R}^N)$ such that $\nabla u_\varepsilon \to \nabla u$ in $L^p((0, 1)^N;{{\mathbb{M}}^{N\times N}})$ and

Specifically, $u$ is a collection of an at most countable family of rigid deformations, i.e., there exists a Caccioppoli partition $\{E_i\}_{i\in\mathbb{N}}$ subordinated to the reduced boundary $\partial^* \{\nabla u \in SO(N)H\}$, such that

where $R_i\in O(N)$ and $b_i\in\mathbb{R}^N$. Moreover, if $\partial^*E_i\cap\partial^*E_j\neq\emptyset$, then $\det R_i \, \det R_j = -1$ and $\partial^*E_i\cap\partial^*E_j$ is flat, i.e., the measure theoretic normal vector to $\partial^*E_i\cap\partial^*E_j$ is constant (up to the sign).

We now prove the main result of this section.

Theorem 2.2. Let $\lambda\in(0, 1)$ and $(P_1, P_2)\in \{ (I, \lambda I), (I, \lambda J) \}$. There exists $C>0$ such that

Moreover,

Proof. The upper bound (2.7) is proven by comparing test functions for $\gamma(P_1, P_2;k)$ with those for $\gamma(P_1, P_2;1)$. Namely, let $v\in A_{\infty}(\Omega _{1, \infty})$ be such that $v(x) = P_1Hx$ for every $x\in \mathcal{L}_\infty^-(k)$ and $v(x) = P_2Hx$ for every $x\in \mathcal{L}_\infty^+(k)$; in particular, $\nabla v = P_1H$ for $x_1\in (-\infty, -1)$ and $\nabla v = P_2 H$ for $x_1\in(0, +\infty)$. Then one defines $u\in \mathcal{A}_{\infty}(\Omega _{k, \infty})$ by $u(x) : = k v(x/k)$, which yields $\gamma(P_1, P_2;k) \leq \mathcal{E} _{\infty }^{1, \lambda }(u, k) \leq C \, \mathcal{E} _{\infty }^{1, \lambda }(v, 1) \, k^N$, and thus $\gamma(P_1, P_2;k) \leq C \, \gamma(P_1, P_2;1)\, k^N$. Note that in the previous inequalities one uses the fact that $\nabla v\in L^{\infty}$ and that the energy of the interactions in $B_2$ can be bounded, using the Mean Value Theorem, by the energy of the interactions in $B_1$.

For the proof of the lower bound (2.8) we will use Theorem 2.1 in each of the subsets $(-1, 0) \times (-1, 1)^{N-1}$ and $(0, 1) \times (-1, 1)^{N-1}$. By contradiction, suppose that there exist a sequence $k_j\nearrow\infty$ and a sequence $\{u_j\}\subset \mathcal{A}_{\infty}(\Omega _{k_j, \infty})$ such that

for some positive $C$. Define $v_j\colon\Omega _{1, \infty}\to \mathbb{R}^N$ as $v_j(x) : = \frac{1}{k_j} u_j(k_j x)$. Accordingly, we consider the rescaled lattices

Expressing $\mathcal{E} _{\infty }^{1, \lambda }(u_j, k_j)$ in terms of $v_j$, one finds

The above term controls the (piecewise constant) gradient of $v_j$. From (2.9), (2.10), and Theorem 2.1 we deduce that, up to subsequences, $\nabla v_j \to \nabla v$ in $L^p((-1, 1)^{N};{{\mathbb{M}}^{N\times N}})$, for some $v\in W^{1, \infty}((-1, 1)^N;\mathbb{R}^N)$, where $\nabla v\in O(N)H$ for a.e. $x\in (-1, 0) \times (-1, 1)^{N-1}$ and $\nabla v\in \lambda\, O(N)H$ for a.e. $x\in (0, 1) \times (-1, 1)^{N-1}$. Precisely,

where $R_i, Q_j \in O(N)$, $a_i, b_j\in\mathbb{R}^N$, and $\{E_i^-\}$ (respectively $\{E_j^+\}$) is a Caccioppoli partition of $(-1, 0) \times (-1, 1)^{N-1}$ (respectively of $(0, 1) \times (-1, 1)^{N-1}$). Then, since $\{E_i^-\} \cup \{E_j^+\}$ is a Caccioppoli partition of $(-1, 1)^N$, by the local structure of Caccioppoli partitions (see e.g. [3,Theorem 4.17]), we find that, for $\mathcal{H}^{N-1}$-a.e. $x\in \{0\}{\times}(-k, k)^{N-1}$, $x\in \partial^* E^-_i \cap \partial^* E^+_j$ for some $i, j$ (where $\partial^* E$ denotes the reduced boundary of $E$). Therefore, using a blow-up argument and the fact that $v\in W^{1, \infty}((-1, 1)^N;\mathbb{R}^N)$, we deduce that there exist rank-1 connections between $O(N)H$ and $\lambda\, O(N)H$; see [2,Lemma 3.2]. This implies in particular that $\lambda = 1$, which is a contradiction to $\lambda\in(0, 1)$. Hence (2.8) follows.

Remark 1. An estimate similar to (2.8) was proven in [14,15] (for a hexagonal lattice in dimension two and a class of three-dimensional lattices) via a different argument, based on the non-interpenetration condition. In fact, in [14,15] a stronger result is proven, namely, that $\gamma (I, \lambda I;k)$ scales like $k^N$.

The non-interpenetration assumption turns out to be necessary if the energy involves only nearest neighbour interactions; indeed, in such a case, one can exhibit deformations that violate the non-interpenetration condition and for which (2.8) does not hold, see [14,Section 4.2]. Such deformations, which consist of suitable foldings of the lattice, would be energetically expensive (and, in particular, would not provide a counterexample to (2.8)) in the present setting, exactly because of the effect of the interactions across neighbouring cells. It is the latter ones that prevent folding phenomena and allow one to prove (2.8), via Theorem 2.1.

3.   Compactness and lower bound

Before characterising the $\Gamma$-convergence for the rescaled functionals (1.7), we show a compactness theorem for sequences with equibounded energy, as well as bounds from above and from below on those functionals in terms of the changes of orientation in the wire. Such bounds will be used in the proof of the $\Gamma$-convergence results, Theorems 5.1 and 5.4.

Essential tools for the compactness and the lower bound are provided by the following rigidity estimates.

Theorem 3.1. [12,Theorem 3.1] Let $N\geq 2$, and let $1 < p < \infty$. Suppose that $U\subset\mathbb{R}^{N}$ is a bounded Lipschitz domain. Then there exists a constant $C = C(U)$ such that for each $u\in W^{1, p}(U;\mathbb{R}^{N})$ there exists a constant matrix $R\in SO(N)$ such that

The constant $C(U)$ is invariant under dilation and translation of the domain.

It is convenient to define the energy of a single simplex $T$ with vertices $x_0, \dots, x_N$,

where $u_F$ is the affine map $u_F(x): = Fx$. The following lemma provides a lower bound on ${E_{{\rm{cell}}}}(u_F;T)$ in terms of the distance of $F$ from $O(N)$. It will be instrumental in using Theorem 3.1.

Lemma 3.2. [2,Lemma 2.2] There exists a constant $C>0$ such that

The next lemma asserts that if in two neighbouring simplices the sign of $\det \nabla u$ has different sign, then the energy of those two simplices is larger than a positive constant. It will be convenient to define the energetic contribution of the interactions within two neighbouring simplices $T = [x_0, x_1, \dots, x_N]$, $S = [y_0, x_1, \dots, x_N]$ as

Lemma 3.3. [2,Lemma 2.3] There exists a positive constant $C_0$ (depending on $H$) with the following property: if two neighbouring $N$-simplices $S$, $T$ have different orientations in the deformed configuration, i.e.,

then ${E_{{\rm{cell}}}}(u;S\cup T)\ge C_0$.

Lemma 3.2 will allow us to apply Theorem 3.1. More precisely, in the part of the wire with $x_1\in(-L, 0)$ we use (3.1) or its "symmetric" version for $O(N){\setminus}SO(N)$ in subdomains that scale in such a way that the constant of the rigidity estimate does not change; for $x_1\in(0, L)$ we use corresponding estimates for $\lambda\, SO(N)$ or $\lambda(O(N){\setminus}SO(N))$. Thus we approximate the deformation gradient with piecewise constant matrices in $O(N)$, respectively $\lambda\, O(N)$.

Due to the fact that a minimum energy has to be paid for each change of orientation, see Lemma 3.3, the parts with positive determinant do not mix with those with negative determinant. Hence, passing to the weak* limit we obtain functions taking values in ${\rm{co}}(SO(N)) \cup {\rm{co}}(O(N) {\setminus} SO(N))$, respectively $\lambda\, {\rm{co}}(SO(N)) \cup \lambda\, {\rm{co}}(O(N) {\setminus} SO(N))$. Here, ${\rm{co}}(X)$ denotes the convex hull of a set $X$ in ${{\mathbb{M}}^{N\times N}}$.

Remark 2. It is well known that ${\rm{co}}(SO(N)) \cap {\rm{co}}(O(N) {\setminus} SO(N)) \neq\emptyset$: indeed, the intersection always contains the zero matrix, here denoted by $0$. In dimension $N = 2$, one can see that

In particular, ${\rm{co}}(SO(2)) \cap {\rm{co}}(O(2) {\setminus} SO(2)) = \{0\}$. For $N>2$, the intersection is nontrivial. For example, ${\rm{co}}(SO(3)) \cap {\rm{co}}(O(3) {\setminus} SO(3))$ contains the matrix $-\frac13I$. Moreover, one can see that

for $N\ge2$.

Henceforth, the symbol $\mathcal{U}$ stands for the class of subsets of $(-L, L)$ that are disjoint union of a finite number of open intervals.

Proposition 2. Let ${\tilde{u}}_\varepsilon\in {\tilde {\mathcal{A}}}_{\varepsilon}(\Omega _{k})$ be a sequence such that

Then there exist functions ${\tilde{u}} \in W^{1, \infty}(\Omega _k;\mathbb{R}^N)$, $d_1, \dots, d_N\in L^{\infty}(\Omega _k;\mathbb{R}^N)$, and a subsequence (not relabelled) such that

and ${\tilde{u}}$, $d_1, \dots, d_N$, are independent of $x_2, \dots, x_N$, i.e., $\partial_{j}{\tilde{u}} = \partial_{j} d_i = 0$, for each $i = 2, \dots, N$ and $j = 2, \dots, N$. Moreover, there exists $U\in\mathcal{U}$ such that

and

Remark 3. The right-hand side of (3.6) contains different contributions. The first term corresponds to the minimal energy needed to bridge a rotation with a rotoreflection, or viceversa, in the left part of the nanowire; the energy spent depends on the number of changes of orientation, i.e., on the cardinality of $\partial U$. The second term plays an analogous role for the right part of the nanowire. The remaining terms describe the interfacial energy spent to bridge the two energy wells $O(N)H$ and $\lambda\, O(N)H$: that contribution also depends on whether or not the orientation is preserved across the interface, i.e., on whether $0$ is an inner or external, or boundary point for $U$.

Proof. (Compactness) The assumption (3.3) implies that $\{\nabla u_\varepsilon\}$, resp. $\{\nabla {\tilde{u}}_\varepsilon A_\varepsilon^{-1}\}$, is uniformly bounded in $L^{\infty}(\Omega _k\varepsilon ;{{\mathbb{M}}^{N\times N}})$, respectively $L^{\infty}(\Omega _k;{{\mathbb{M}}^{N\times N}})$. (Recall that $u_\varepsilon(x) = \tilde{u}_\varepsilon(A_\varepsilon^{-1} x)$.) Therefore there exist a subsequence of $\{{\tilde{u}}_\varepsilon\}$ (not relabelled) and functions ${\tilde{u}}\in W^{1, \infty}(\Omega _k;\mathbb{R}^N)$ and $d_i \in L^{\infty}(\Omega _k;\mathbb{R}^N)$ for $i = 2, \dots, N$, such that $\partial_{1}{\tilde{u}}_\varepsilon \mathop * \limits_ \rightharpoonup \partial_{1} {\tilde{u}}$ weakly^* in $L^{\infty}(\Omega _k;{{\mathbb{M}}^{N\times N}})$, where ${\tilde{u}}$ is independent of $x_i$ for all $i = 2, \dots, N$, and $\frac{1}\varepsilon\partial_{i}{\tilde{u}}_\varepsilon \mathop * \limits_ \rightharpoonup d_i$ for each $i = 2, \dots, N$.

In order to show $\partial_{j}d_i = 0$ and (3.5), we apply the rigidity estimate (3.1) to the sequence $u_\varepsilon$. To this aim, we divide the domain $\overline{\Omega}_{k\varepsilon}$ into subdomains that are the Cartesian product of intervals $(a_i, a_i +\varepsilon)$, $a_i\in\varepsilon\mathbb{Z}$, and the cross-section $(k\varepsilon, k\varepsilon)^{N-1}$. We first observe that, by Lemma 3.3 and assumption (3.3), the number of changes of orientation of $u_\varepsilon$ is uniformly bounded in $\varepsilon$. More precisely, we can find a uniformly bounded number of subdomains $(a_i, a_i +\varepsilon)\times(k\varepsilon, k\varepsilon)^{N-1}$, $i\in I_\varepsilon$, $\# I_\varepsilon \le C$, such that if $i\notin I_\varepsilon$ then $\det\nabla u_\varepsilon$ has constant sign in $(a_i, a_i +\varepsilon)\times(k\varepsilon, k\varepsilon)^{N-1}$. In each of these subdomains, we use (3.2) to apply the rigidity estimate (3.1), or its "symmetric" version for $O(N){\setminus}SO(N)$.

Specifically, for each $a_i$ with $a_i < 0$ and $i\notin I_\varepsilon$, there exists $P_\varepsilon (a_i)\in O(N)H$ such that

and for every $a_i >0$ with $i\notin I_\varepsilon$ there exists $P_\varepsilon (a_i)\in \lambda \, O(N) H$ such that

Moreover for $i\in I_\varepsilon$ we set $P_\varepsilon(a_i) = I$ if $a_i <0$ and $P_\varepsilon(a_i) = \lambda I$ if $a_i\ge0$. By interpolation one defines a piecewise constant matrix field $P_\varepsilon:(-L, L)\to O(N)H \cup \lambda \, O(N) H$ such that $P_\varepsilon(x_{1}) = P_\varepsilon(a_i)$ if $x_{1}\in (a_i, a_i+\varepsilon)$. Summing up over $i$ and rescaling the variables, one gets

where the last inequality of each line follows by applying Lemma 3.2 to each subdomain with $i\notin I_\varepsilon$ and by recalling that each subdomain has volume proportional to $\varepsilon$ after rescaling.

We now define the sets

and remark that Lemma 3.2, Lemma 3.3, and assumption (3.3) imply that the cardinality of $\partial U_\varepsilon$ is uniformly bounded. Therefore the sequence $\{\chi_{U_\varepsilon}\}$ converges, up to subsequences, to $\chi_{U}$ strongly in $L^1(-L, L)$, where

Since we can write

where $R_\varepsilon : (-L, L) \to SO(N)$ is piecewise constant, we deduce that $P_\varepsilon$ converges, up to subsequences, to some $P\in L^\infty((-L, L);{{\mathbb{M}}^{N\times N}})$ in the weak^* topology of $L^\infty((-L, L);{{\mathbb{M}}^{N\times N}})$. From (3.7) it follows that the weak* limit of $\nabla {\tilde{u}}_\varepsilon A_\varepsilon^{-1}$ coincides with $P$ and therefore does not depend on $x_j$ for each $j = 2, \dots, N$. Moreover, inclusion (3.5) follows from the fact that $\chi_{U_\varepsilon}P_\varepsilon$ converges weakly^* to $\chi_{U}P$.

(Lower bound) Inequality (3.6) is proven by a standard argument which can be found, for example, in [14,16,17]. We will briefly sketch the main ideas and refer the reader to [14,16,17] for full details. First recall that $\partial U$ consists of a finite number of points, cf. (3.8). Since $\chi_{U_\varepsilon} \to \chi_U$ and since the number of points of $\partial U_\varepsilon$ is uniformly bounded, one can find $\sigma >0$, $\alpha_i^\varepsilon \to \alpha_i$, $\beta_i^\varepsilon \to \beta_i$ such that

Moreover, if $\sigma$ is sufficiently small, all the intervals $(\alpha_i^\varepsilon -2\sigma, \alpha_i^\varepsilon + 2 \sigma )$ and $(\beta_i^\varepsilon -2\sigma, \beta_i^\varepsilon + 2 \sigma )$ are mutually disjoint and therefore it suffices to prove the lower bound for one of such intervals. Suppose that $\alpha_i^\varepsilon \in (0, L)$ and define

Then, $\nabla v_\varepsilon (x) = \nabla {\tilde{u}}_\varepsilon (\varepsilon x_1 + \alpha_i^\varepsilon, x_2, \dots, x_N) A_\varepsilon^{-1} = \nabla u_\varepsilon(\varepsilon x_1 + \alpha_i^\varepsilon, \varepsilon x_2, \dots, \varepsilon x_N)$, and, by (3.7), we have

From (3.10), Theorem 3.1 and the Poincaré inequality, we deduce that there exists a unit interval contained in $(-\frac{2\sigma}\varepsilon, -\frac{\sigma}\varepsilon)$ such that in the Cartesian product of such interval with the cross-section $(-k, k)^{N-1}$, the $W^{1, p}$-norm of the difference between $v_\varepsilon$ and an affine map of the form $\lambda Q H x + a$, with $Q\in O(N){\setminus}SO(N)$ and $a\in \mathbb{R}^N$, is bounded by $C \varepsilon/\sigma$. By the same argument one can find a unit interval contained in $(\frac{\sigma}\varepsilon, \frac{2\sigma}\varepsilon)$ such that in the Cartesian product of such interval with the cross-section $(-k, k)^{N-1}$, the $W^{1, p}$-norm of the difference between $v_\varepsilon$ and an affine map of the form $\lambda RH x + b$, with $R\in SO(N)$ and $b\in \mathbb{R}^N$, is bounded by $C \varepsilon/\sigma$. By gluing the function $v_\varepsilon$ with these maps on such intervals, one can define a function $\hat{v}_\varepsilon\in \mathcal{A}_{\infty}(\Omega _{k, \infty})$ that is a competitor for $\gamma (\lambda J, \lambda I;k)$ and such that (cf.(2.2))

where $\mathcal{I}_{\varepsilon }^{1,\lambda } (\tilde u_\varepsilon, k)|_{(\alpha_i^\varepsilon -2\sigma, \alpha_i^\varepsilon + 2\sigma )\times (-k, k)^{N-1}}$ only takes into account the interactions between atoms lying in the subset $(\alpha_i^\varepsilon -2\sigma, \alpha_i^\varepsilon + 2\sigma )\times (-k, k)^{N-1}$. Arguing in a similar way for the other intervals in (3.9) yields (3.6).

4.   Upper bound

We prove that the bound (3.6) is in fact optimal.

Proposition 3. Let $F\in L^{\infty}((-L, L);{{\mathbb{M}}^{N\times N}})$ and $U\in\mathcal{U}$ satisfy

Then there exists a sequence $\{{\tilde{u}}_\varepsilon\}\subset {\tilde {\mathcal{A}}}_{\varepsilon}(\Omega _{k})$ such that

and

Proof. Using a standard approximation argument we may assume that $x_1\mapsto F(x_1)$ is piecewise constant, with values in $O(N)H$ for a.e. $x_1\in(-L, 0)$ and values in $\lambda\, O(N)H$ for a.e. $x_1\in(0, L)$. We may also assume that this approximation process does not modify the set $U$ of (4.1). More precisely, there exist $m, n\in\mathbb{Z}$, $m < 0$, $n\ge0$, $-L = a_m < a_{m+1} < \dots < a_{-1} < a_0 = 0 < a_1 < \dots < a_n < a_{n+1} = L$, and $R_{i}\in O(N)$ for $i = m, \dots, -1, 0, \dots, n$ such that

and

The following construction is similar to that in [14,Proposition 3.2], so we will show the details only for what concerns the changes of orientation. We introduce a mesoscale $\{\sigma_\varepsilon\}$ such that $\varepsilon \ll\sigma_\varepsilon\ll 1$ as $\varepsilon\to0^+$. Next we define $\tilde u_\varepsilon$ in the sets of the type $(a_i{+}\sigma_\varepsilon, a_{i+1}{-}\sigma_\varepsilon)\times(-k, k)^{N-1}$ in such a way that its gradient equals $R_i H A_\varepsilon$ if $a_{i+1}\le0$ and equals $\lambda R_i H A_\varepsilon$ if $a_i\ge 0$. This determines $\tilde u_\varepsilon$ in those regions, up to some additive constants that will have to be fixed at the end of the construction in order to make $\tilde u_\varepsilon$ continuous.

We now complete the definition of $\tilde u_\varepsilon$ in the sets of the type $(a_i{-}\sigma_\varepsilon, a_{i}{+}\sigma_\varepsilon)\times(-k, k)^{N-1}$. Let us first assume $i < 0$, i.e., $a_i < 0$. Since $R_{i-1}$ and $R_{i}$ may be in $SO(N)$ or in $O(N){\setminus} SO(N)$, one can have four cases. If both $R_{i-1}$ and $R_i$ are in $SO(N)$, it is possible to define $\tilde u_\varepsilon$ by interpolating $R_{i-1}$ and $R_i$ so that the cost of the transition has order $O(\varepsilon/\sigma_\varepsilon)$, so it gives no contribution to (4.3); we refer to [14] for details. The case $R_{i-1}, R_i\in O(N){\setminus} SO(N)$ is completely analogous.

If $R_{i-1}\in SO(N)$ and $R_i\in O(N){\setminus} SO(N)$ or viceversa, we define $\tilde u_\varepsilon$ in the set $(a_i{-}\sigma_\varepsilon, a_{i}{+}\sigma_\varepsilon)\times(-k, k)^{N-1}$ as a rescaling of a quasiminimiser of (2.1b). More precisely, we fix $\eta>0$ and apply the definition of $\gamma (R_{i-1}, R_i;k)$, thus finding $M>0$ and $v\in \mathcal{A}_{\infty}(\Omega _{k, \infty})$ such that

and

where we used also Proposition 1. With this at hand, we define $\tilde u_\varepsilon$ in the set $(a_i{-}\sigma_\varepsilon, a_{i}{+}\sigma_\varepsilon)\times(-k, k)^{N-1}$ as

The constant vector $b$ in the last equation is chosen in such a way that $\tilde u_\varepsilon$ is continuous. Since each point of $\partial U$ gives the same contribution $\gamma (I, J;k)$ to the upper bound, we obtain the first term of (4.3).

The case $i>0$, i.e., $a_i>0$, is treated similarly to $i < 0$ and gives rise to the second term of (4.3). Finally, for $i = 0$, i.e., $a_i = a_0 = 0$, we argue as above and define $\tilde u_\varepsilon$ by using a rescaling of a quasiminimiser of (2.1a) and applying the definition of $\gamma (R_{-1}, \lambda R_0;k)$. We then get an interfacial contribution in (4.3) that differs in the two cases $0\in \partial U$ and $0\notin\partial U$.

5.   Limit functionals with respect to different topologies

In the next theorem we characterise the $\Gamma$-limit of the sequence $\{ \mathcal{I}_{\varepsilon }^{1,\lambda }(\cdot, k) \}$ with respect to the weak* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)$; see [4,8] for an introduction to $\Gamma$-convergence. As it can be inferred from the compactness result in Proposition 2, the domain of the $\Gamma$-limit turns out to be

We show that on such domain the $\Gamma$-limit is constant. Hence, the macroscopic description of the model is similar to that of [14,15]; in particular, it does not have memory of the changes of orientation in minimising sequences. In order to keep track of the orientation changes, we need to introduce a stronger topology for the $\Gamma$-convergence, as we see in Theorem 5.4.

Theorem 5.1. The sequence of functionals $\{ \mathcal{I}_{\varepsilon }^{1, \lambda }(\cdot, k)\}$ $\Gamma$-converges, as $\varepsilon\to 0^{+}$, to the functional

with respect to the weak^* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)$, where

Proof. (Liminf inequality) Let ${\tilde{u}}_\varepsilon \in {\tilde {\mathcal{A}}}_{\varepsilon}(\Omega _{k})$ be a sequence of functions converging to a function $u$ weakly^* in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)$. We have to show that

We assume that $\liminf_{\varepsilon \to 0^+} \mathcal{I}_{\varepsilon }^{1,\lambda }({\tilde{u}}_\varepsilon, k) \le C$, the other case being trivial. By applying Proposition 2 we find a set $U\in\mathcal{U}$ and functions ${\tilde{u}} \in W^{1, \infty}(\Omega _k;\mathbb{R}^N)$, $d_2, \dots, d_N\in L^{\infty}(\Omega _k;\mathbb{R}^N)$ independent of $x_2, \dots, x_N$, such that (3.4), (3.5), and (3.6) hold. This implies that $\partial_1u = \partial_1{\tilde{u}}$ a.e., the function $u$ is independent of $x_2, \dots, x_N$, and $u\in \mathcal{A}^{1,\lambda }(k)$. Notice that the right-hand side of (3.6) is greater than or equal to $\gamma(k)$, since $\gamma(\cdot, \cdot;k)$ is positive.

(Limsup inequality) Given a function $u\in W^{1, \infty}(\Omega _k;\mathbb{R}^N)$ we have to find a sequence $\{{\tilde{u}}_\varepsilon\}\subset {\tilde {\mathcal{A}}}_{\varepsilon}(\Omega _{k})$ such that ${\tilde{u}}_\varepsilon \mathop * \limits_ \rightharpoonup u$ weakly^* in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)$ and

We assume that $u\in\mathcal{A}^{1,\lambda }(k)$, the other case being trivial.

The construction of the recovery sequence depends on the precise value of the minimum in (5.3). Since we do not know such value, we explain how to proceed in the case when $\gamma(k)$ is any of the two quantities therein.

$\bullet$ If $\gamma(k) = \gamma(I, \lambda I;k)$, we set $U: = (-L, L)$ and, following e.g. [16,Theorem 4.1], we construct measurable functions $d_{2}, \dots, d_N\in L^{\infty}(\Omega _k;\mathbb{R}^{N})$, independent of $x_2, \dots, x_N$, such that

$\bullet$ If $\gamma(k) = \gamma(I, \lambda J;k)$ we set $U: = (-L, 0)$ and construct $d_{2}, \dots, d_N$ in such a way that

Proposition 3 can be now applied to $F: = (\partial_1 u \, | \, d_2 \, | \, \cdots \, | \, d_N)$, hence providing us with a sequence $\{{\tilde{u}}_\varepsilon\}\subset {\tilde {\mathcal{A}}}_{\varepsilon}(\Omega _{k})$ satisfying (4.2)-(4.3). In particular we have $\nabla{\tilde{u}}_\varepsilon \mathop * \limits_ \rightharpoonup \nabla u$ weakly^* in $L^{\infty}(\Omega _k;{{\mathbb{M}}^{N\times N}})$ and (5.4) holds because of the choice of $U$ and the definition of $\gamma(k)$.

Remark 4. As long as the $\Gamma$-convergence is taken with respect to the weak* topology of $W^{1, \infty}(\Omega _k;\mathbb{R}^N)$, (5.2) only accounts for the cost of transitions at the interface between the two species of atoms. Indeed, away from the interface it is always possible to construct recovery sequences without mixing rotations and rotoreflections, as done in the proof of the limsup inequality; such transitions have low interaction energy, since $\gamma(I, I) = \gamma(J, J) = 0$, see also Proposition 1. In particular, for $\lambda = 1$ the limit functional is trivial, since $\mathcal{I}^{1,1}(u, k) = 0$ if $u\in\mathcal{A}^{1,1}(k)$.

Below we show that, if a stronger topology is chosen, the value of the $\Gamma$-limit changes. The resulting limit functional depends on an internal variable, $D$ in (5.7), that keeps track of the changes of orientation throughout the thin wire. In fact, different transitions between the energy wells must now be employed according to the value of $D$; two examples are provided in Figure 2.

We introduce the sequence of functionals defined for $u\in W^{1, \infty}(\Omega _k;\mathbb{R}^N)$ and $D\in L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$ by

In the next theorem we study the $\Gamma$-limit of the sequence $\left\{ {\widehat {\cal I}_\varepsilon ^{1,\lambda }( \cdot , \cdot ,k)} \right\}$ as $\varepsilon\to0^+$ with respect to the weak* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)\times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$. As a consequence of Proposition 2, the domain of the $\Gamma$-limit turns out to be

where $\mathcal{A}^{1,\lambda }(k)$ is defined by (5.1). It is convenient to introduce the following definition, where the functional $\mathcal{J}$ coincides with the right-hand sides of (3.6) and (4.3).

Definition 5.2. Given $(u,D) \in {\widehat {\cal A}^{1,\lambda }}(k)$, let $\mathcal{U}(u, D)$ be the collection of all subsets $U\in\mathcal{U}$ such that

For $U\in\mathcal{U}(u, D)$ we set

and

The last definition will be used to apply Propositions 2 and 3 towards the characterisation of the $\Gamma$-limit with respect to the stronger topology. To this end, each pair $(u,D)\in {{\widehat{\mathcal{A}}}^{1,\lambda }}(k)$ is associated with a set $U$ realising (5.5). Such $U$ is in general not unique, since ${\rm{co}}(SO(N)) \cap {\rm{co}}(O(N){\setminus} SO(N)) \neq \emptyset$. Therefore, we choose it to be "optimal", i.e., minimising (5.6). Notice that the minimum in (5.6) is attained since

A minimiser needs not be unique as shown in the following example.

Example 5.3. Fix $a_1 < a_2 < 0$ and assume that $D(x_1)\in (O(N){\setminus}SO(N))H$ for $x_1 < a_1$, $D(x_1) = 0$ for $a_1 < x_1 < a_2$, $D(x_1)\in SO(N)H$ for $a_2 < x_1 < 0$, and $D(x_1)\in \lambda\, SO(N)H$ for $x_1>0$. Then any interval of the type $U = (a, +\infty)$, with $a_1\le a\le a_2$, is a minimiser of (5.6).

Theorem 5.4. The sequence of functionals $\{\widehat{\mathcal{I}}_{\varepsilon }^{1,\lambda }(\cdot ,\cdot ,k)\}$ $\Gamma$-converges, as $\varepsilon\to 0^{+}$, to the functional

with respect to the weak^* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)\times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$, where ${\mathcal{J}_{\min }}(u, D)$ is defined by (5.6).

Proof. The liminf inequality is obtained by applying Proposition 2 and arguing as in Theorem 5.1. Also the derivation of the limsup inequality is similar to the one performed in Theorem 5.1; let us simply point out that, while in the proof of Theorem 5.1 the matrix field $F$ needed to be reconstructed, here we set $F: = D$ and choose $U$ as a minimiser of (5.6). The conclusion follows by applying Proposition 3.

Remark 5. We underline that Theorem 5.4 provides a nontrivial $\Gamma$-limit also in the case when $\lambda = 1$. Indeed, one has ${{\widehat{\mathcal{I}}}^{1,1}}(u,D,k)=\gamma (I,J;k){{\mathcal{H}}^{0}}(\partial U\cap (-L,L))$ if $(u,D)\in {{\widehat{\mathcal{A}}}^{1,1}}(k)$ and $U$ miminises (5.6), where $\gamma (I, J;k)>0$.

6.   Boundary conditions and external forces

In the present section we discuss how the previous results extend to the case when the functional (1.4) is complemented by boundary conditions or external forces. Although our considerations apply to the case of general $H\in GL^+(N)$ and $\lambda \in (0, 1]$, for simplicity we will focus on the case $H = I$ and $\lambda = 1$. We will also test the consistency of the present model with the non-interpenetration condition by looking at minimisers of the $\Gamma$-limit when boundary conditions or forces are prescribed. We will see that the continuum limit that keeps track of such constraints is the one provided by the stronger topology (5.7).

Boundary conditions. Let $B^-, B^+\in GL^+(N)$ and suppose that the functional (1.4) is now defined on deformations $u\in\mathcal{A}_{\varepsilon}(\Omega _k\varepsilon )$ that satisfy

It is easy to see that while the compactness result of Proposition 2 remains valid, the $\Gamma$-limit (5.2) will now contain additional terms corresponding to the minimal energy spent to fix the atoms in the vicinity of the lateral boundaries. However, such extra terms do not depend on the limiting deformations, therefore they do not encode any information about the behaviour of minimising sequences. As far as the stronger topology is concerned, one can see that the limit functional (5.7) will contain the additional quantities $\gamma (B^-, P;k)$ and $\gamma (P, B^+;k)$ defined, for $P\in\{I, J\}$, by

where $\mathcal{E} _M^{1,1}$ is as in (2.1b), except that the sum is taken over all atoms contained in the bounded strip $(-M, M)\times (-k, k)^{N-1}$. The choice of $P = I$ or $P = J$ depends on whether or not $\pm L \in \partial \bar U$, where $\bar U$ is a minimiser of (5.6). Precisely, if $-L \in \partial \bar U$ (resp. $L \in \partial \bar U$), then in (6.2) (resp. (6.3)) we take $P = I$, otherwise we take $P = J$.

Remark 6. By Proposition 2 and the properties of $\Gamma$-convergence, minimisers of (1.4) subjected to (6.1) converge, up to subsequences, to minimisers of (5.7) complemented with the above extra terms. Moreover, if $\text{dist}(B^{\pm};SO(N))$ is sufficiently small, then such minimisers will not have transitions between $\text{co}\big(SO(N)\big)$ and $\text{co}\big(O(N){\setminus} SO(N)\big)$. This follows from the fact that

and therefore, as long as $\gamma(I, B^{+};k)+\gamma(B^{-}, I;k) < \gamma(I, J;k)$, the optimal transitions will fulfil the non-interpenetration condition. In this respect the quantity $\gamma(I, J;k)$ can be regarded as an energetic barrier that must be overcome in order to have folding effects.

External forces. We study a class of tangential/radial forces acting along the rod. Let $F_1\in \mathbb{R}^N$, $F_2, \dots, F_{N}\in C^0(\mathbb{R}^N;\mathbb{R}^N)$ be a collection of vector fields such that $F_i = F_i(x_1)$ for every $2 = 1, \dots, N$. We denote by $F$ the matrix field whose columns are $F_1, \dots, F_N$. For each $u \colon\mathcal{L}_\varepsilon(k)\to\mathbb{R}^N$, consider the functional

where $L_\varepsilon: = L$ if $L$ is an integer multiple of $\varepsilon$, and $L_\varepsilon: = ([L/\varepsilon] +1)\varepsilon$ otherwise. The functional $\mathcal{F}_\varepsilon$ consists of several terms: the first sum represents a tangential force, while the other terms define a radial force acting on the external atoms of the lattice and enforcing the average displacements along the coordinate directions $e_2, \dots, e_N$ to be aligned with the given vector fields $F_2, \dots, F_{N}$. Note that $\mathcal{F}_\varepsilon(u, k)$ can be written as

hence we have that $\mathcal{F}_\varepsilon(u, k)\simeq\frac{1}{\varepsilon^{N-1}}\int {\Omega _{k\varepsilon}}{F:\nabla u}{\rm{d}}x$.

Introducing the new variables $z(x): = A_\varepsilon x$ defined by (1.6), and adopting the notation used in Section 1, (6.4) can be equivalently expressed in terms of ${\tilde{u}}(x) : = u(z(x))$, namely

so that ${\tilde{\mathcal{F}}}_\varepsilon({\tilde{u}}, k)\simeq \int {\Omega _{k}}{F:(\nabla {\tilde{u}}\, A_\varepsilon^{-1})}{\rm{d}}{x}$. We can then address the study of the asymptotic behaviour of the sequence

Note that in this context we cannot use the weak^* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)$, since this does not control ${\tilde{\mathcal{F}}}_\varepsilon({\tilde{u}})$, which is in fact a term depending on $D = \nabla{\tilde{u}}\, A_\varepsilon^{-1}$. This justifies the choice of $\widehat{\mathcal{I}}_{\varepsilon }^{1,1}$ rather than $\mathcal{I}^{1,1}_\varepsilon$ in the definition of $\mathcal{G}_\varepsilon$: in order to control both terms in the right hand side of (6.5), we use the stronger topology provided by the weak* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)\times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$. The force term is indeed a continuous perturbation of $\widehat{\mathcal{I}}_{\varepsilon }^{1,1}$ with respect to such topology. We observe that

and

Let now $\{({\tilde{u}}_\varepsilon, D_\varepsilon)\} \in {\tilde {\mathcal{A}}}_\varepsilon(\Omega _{k}) \times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$ be a sequence such that

The previous inequalities imply that $|| \nabla {\tilde{u}}\, A_\varepsilon^{-1} ||_{L^p(\Omega _k;{{\mathbb{M}}^{N\times N}})}$ is equibounded, which in turn implies that $\limsup_{\varepsilon\to 0^{+}} \widehat{\mathcal{I}}_{\varepsilon }^{1,1}({\tilde{u}}_\varepsilon, k) \leq C$ and thus the conclusions of Proposition 2 are still valid. (See also [16,Remark 4.2] for similar results.) Taking also into account Theorem 5.4, we derive the following result.

Theorem 6.1. The following results hold:

(Compactness) Let $\{({\tilde{u}}_\varepsilon, D_\varepsilon)\} \in {\tilde {\mathcal{A}}}_\varepsilon(\Omega _{k}) \times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$ be a sequence such that

Then there exists $(\tilde{u},D)\in {{\widehat{\mathcal{A}}}^{1,1}}(k)$ and a subsequence (not relabelled) such that

($\Gamma$-limit) The sequence of functionals $\{ \mathcal{G}_\varepsilon \}$ $\Gamma$-converges, as $\varepsilon\to 0^{+}$, to the functional

with respect to the weak^* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)\times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$, where

for $D{ = }(d_1| \cdots | d_N)$.

As a consequence of the previous theorem and the standard properties of $\Gamma$-convergence we infer the following result about convergence of minima and minimisers.

Corollary 1. We have that

Moreover if $(u_\varepsilon, D_\varepsilon)\in {\tilde {\mathcal{A}}}_\varepsilon(\Omega _{k}) \times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$ is such that

then any cluster point $(\overline u, \overline D)$ of $(u_\varepsilon, D_\varepsilon)$ with respect to the weak^* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)\times L^\infty(\Omega _k;{{\mathbb{M}}^{N\times N}})$ is a minimiser for $\min \{\mathcal{G}(u,D,k):(u,D)\in {{\widehat{\mathcal{A}}}^{1,1}}(k)\}$.

We now come back to the question of the consistency of the model with the non-interpenetration condition. In this context we cannot expect that minimisers of (6.5) preserve orientation for the whole class of loads defined above. This is clarified in the following remark.

Remark 7. Minimisers of the functional defined by (6.6) may have transition points between the two wells $SO(N)$ and $O(N){\setminus}SO(N)$. Suppose for instance that $F_1, \dots, F_N$ satisfy the following properties: there exist $n_1, \dots, n_N \in S^{N-1}$, $a\in (-L, L)$, such that $(n_1| \cdots | n_N)\in SO(N)$, $F_i(x_1) = f_{i}(x_1)n_i$ for each $i = 1, \dots, N$, $f_1\in\mathbb{R}$, $f_{i} > 0$ in $(-L, L)$ for each $i = 1, \dots, N-1$, $f_{N} > 0$ in $(-L, a)$, $f_{N} < 0$ in $(a, L)$.

Define $\overline D: = (n_1| \cdots | n_N)$ if $x_1\in(-L, a)$, and $\overline D: = (n_1| \cdots| n_{N-1} | -n_N)$ if $x_1\in(a, L)$. Note that $({{x}_{1}}{{n}_{1}},\bar{D})\in {{\widehat{\mathcal{A}}}^{1,1}}(k)$, and $\overline D$ has a transition point at $x_1 = a$. Denote by $\widehat{\mathcal{A}}_{0}^{1,1}(k)$ the subset of ${{\widehat{\mathcal{A}}}^{1,1}}(k)$ of deformations with no transitions; i.e., $\widehat{\mathcal{A}}_{0}^{1,1}(k):=\{(u,D)\in {{\widehat{\mathcal{A}}}^{1,1}}(k):{{\widehat{\mathcal{I}}}^{1,1}}(u,D,k)=0\}$. It is easy to see that

Therefore, if $f_1, \dots, f_N$ are such that

then it is energetically preferred to have a transition at $a$, namely, all minimisers of $\mathcal{G}$ are given by $(x_1 n_1 + b, \overline D)$, with $b$ any vector in $\mathbb{R}^N$. In contrast, if $f_N$ is always positive, then minimisers will not display any transition.

7.   Comparison with models including dislocations

The lattice mismatch in heterostructured materials, corresponding to $\lambda\neq 1$ in the model described in this section, can be relieved by creation of dislocations; i.e., line defects of the crystal structure. We refer to [9,13,19] for an account of the literature on dislocations in nanowires. A model for discrete heterostructured nanowires accounting for dislocations was studied in [14,15] under the assumption that deformations fulfil the non-interpenetration condition. In this paper we have chosen to consider only defect-free configurations in order to both simplify the exposition and to pose emphasis on the difficulties to overcome when the non-interpenetration assumption is removed. In the final part of the paper, we outline the results that can be obtained when dislocations are accounted for.

Following the ideas of [14], in dimension $N = 2$ we introduce other possible models where the reference configuration represents a lattice with dislocations. More precisely, we fix $\rho\in[\lambda, 1]$ and set

where

and $\overline\Omega _\varepsilon$ is as in (1.1). For $\rho\neq1$, the number of atomic layers parallel to $e_1$ is different in the two sublattices (for sufficiently large $k$); this can be regarded as a system containing dislocations at the interface.

In presence of dislocations, the choice of the interactions and of the equilibria strongly depends on the lattice that one intends to model. Therefore, in this section we focus on the simplest situation of hexagonal (or equilateral triangular) Bravais lattices in dimension two and we fix

The lattice $H \mathcal{L}_\varepsilon(\rho, k)$ consists of two Bravais hexagonal sublattices with different lattice constants $\varepsilon$ and $\rho\varepsilon$, respectively; see Figure 3.

The bonds between nearest and next-to-nearest neighbours are defined first in the lattice $H \mathcal{L}_\varepsilon(\rho, k)$. To this end, one chooses a Delaunay triangulation of $H \mathcal{L}_\varepsilon(\rho, k)$ as defined in [14,Section 1]. Two points $x, y$ of the lattice are said to be nearest neighbours if there is a lattice point $z$ such that the triangle $[x, y, z]$ is an element of the triangulation. Two points $x, y$ are next-to-nearest neighbours if there are $z_1, z_2$ such that $[x, z_1, z_2]$ and $[y, z_1, z_2]$ are elements of the triangulation. These definitions coincide with the usual notions of nearest and next-to-nearest neighbours away from the interface. We underline that other choices of interfacial bonds are possible to derive our main results. Indeed, one may start from any triangulation of the lattice satisfying the following properties: the number of nearest neighbours of each point has to be uniformly bounded by a constant independent of $\varepsilon$, while the length of the bonds in $H \mathcal{L}_\varepsilon(\rho, k)$ has to be uniformly bounded by a constant $C_\varepsilon = C\varepsilon$.

Once the bonds in the lattice $H \mathcal{L}_\varepsilon(\rho, k)$ are defined, we define the bonds of a point $x\in\mathcal{L}_\varepsilon(\rho, k)$ as follows:

We remark that if $x_1\le-2\varepsilon$, then $B_1(x) = B_1$ and $B_2(x) = B_2$, while if $x_1\ge\rho\varepsilon$, then $B_1(x) = \rho B_1$ and $B_2(x) = \rho B_2$, where $B_1, B_2$ are as in (1.2)-(1.3). The total interaction energy is

Notice that away from the interface all bonds in the reference configuration are in equilibrium if $\rho = \lambda$; instead, interfacial bonds are never in equilibrium. The equilibrium distance of two atoms at the interface is in fact an average of the equilibrium distances of the two sublattices. Generalisations of this energy can be considered as described in [14,Section 4].

The results shown in detail in this paper for the defect-free case (corresponding to $\rho = 1$) can be extended to models with dislocations ($\rho\neq1$) without significant changes in the proof. Thus we obtain a $\Gamma$-convergence result for the rescaled functionals $\mathcal{I}_{\varepsilon }^{1, \lambda }(\cdot, \rho, k)$ defined as in (1.7). (Notice that the definition of the admissible functions is given as in the dislocation-free case, with the only variant that the gradients are constant on the elements of the triangulation introduced to define the interfacial bonds.) Before stating the theorem we introduce the lattices

where the triangulation is chosen in analogy with the one for $\mathcal{L}_\varepsilon(\rho, k)$. We also set

with

Theorem 7.1. The sequence of functionals $\{ \mathcal{I}_{\varepsilon }^{1, \lambda }(\cdot, \rho, k)\}$ $\Gamma$-converges, as $\varepsilon\to 0^{+}$, to the functional

with respect to the weak^* convergence in $W^{1, \infty}(\Omega _k;\mathbb{R}^N)$, where

and

The stronger topology introduced in Theorem 5.4 allows us to take into account the cost of "folding" the lattice using rotoreflections, giving deeper insight into deformations that bridge different equilibria. Indeed, it is possible to combine Theorems 5.4 and 7.1 giving the $\Gamma$-convergence in the stronger topology for models with dislocations; we omit the full statement for brevity.

Remark 8. It is easy to see that for $\rho = \lambda$

for some constants $C_1, C_2>0$. To obtain the estimate from above it is sufficient to consider the identical deformation and recall that the maximal length of a bond and the maximal number of bonds per atom in the lattice $\mathcal{L}_{\infty}(\rho, k)$ are uniformly bounded. This configuration corresponds to the case when dislocations are uniformly distributed along the interface between the two sublattices. (Recall that here $N = 2$ and that the length of the interface is $2k$.) In contrast, the cost of a defect-free configuration ($\rho = 1$) is superlinear as already shown in Theorem 2.2. In fact, following the same proof it is possible to conclude that whenever $\rho\neq\lambda$ one has

This gives a mathematical proof of the experimentally observed fact that dislocations are preferred in order to relieve the lattice mismatch when the thickness of the specimen is sufficiently large. We recall that a similar result was proven in [14,15] (under the non-interpenetration assumption), see also Remark 1.

The results sketched here for hexagonal lattices can be obtained also for other lattices by adapting the technique to each specific case. In particular, we refer to [15] for details on the rigidity of face-centred and body-centred cubic lattices in dimension three.