Convergence and Non-convergence of Many-Particle Evolutions with Multiple Signs

We address the question of the convergence of evolving interacting particle systems as the number of particles tends to infinity. We consider two types of particles, called positive and negative. Same-sign particles repel each other, and opposite-sign particles attract each other. The interaction potential is the same for all particles, up to the sign, and has a logarithmic singularity at zero. The central example of such systems is that of dislocations in crystals. Because of the singularity in the interaction potential, the discrete evolution leads to blow-up in finite time. We remedy this situation by regularising the interaction potential at a length-scale δn>0\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$\delta _n>0$$\end{document}, which converges to zero as the number of particles n tends to infinity. We establish two main results. The first one is an evolutionary convergence result showing that the empirical measures of the positive and of the negative particles converge to a solution of a set of coupled PDEs which describe the evolution of their continuum densities. In the setting of dislocations these PDEs are known as the Groma–Balogh equations. In the proof we rely on both the theory of λ\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$\lambda $$\end{document}-convex gradient flows, to establish a quantitative bound on the distance between the empirical measures and the continuum solution to a δn\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$\delta _n$$\end{document}-regularised version of the Groma–Balogh equations, and a priori estimates for the Groma–Balogh equations to pass to the small-regularisation limit in a functional setting based on Orlicz spaces. In order for the quantitative bound not to degenerate too fast in the limit n→∞\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$n \rightarrow \infty $$\end{document} we require δn\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$\delta _n$$\end{document} to converge to zero sufficiently slowly. The second result is a counterexample, demonstrating that if δn\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$\delta _n$$\end{document} converges to zero sufficiently fast, then the limits of the empirical measures of the positive and the negative dislocations do not satisfy the Groma–Balogh equations. These results show how the validity of the Groma–Balogh equations as the limit of many-particle systems depends in a subtle way on the scale at which the singularity of the potential is regularised.


Multi-sign Particle Systems and Dislocations
There is a vast literature on the properties of interacting particle systems, both deterministic and stochastic, as well as on their limits as the number of particles tends to infinity. The most common situation in the rigorous mathematical literature is that of indistinguishable particles. For many systems of this type, especially with bounded interactions, the many-particle limit has been characterised in various ways; see e.g. [12,43,56,63,64] for reviews. For unbounded interaction forces the situation is more delicate, and rigorous proofs of convergence are more recent [2,16,17,33,40,50,54,58,60,68,69].
In this paper we study a type of particle system that is less intensively studied: a system with two species, called positive and negative particles [8,19,21,29,30,65]. In our setting, we also consider singular interactions. Such systems arise naturally as models of the evolution of dislocations in crystals. Since this example is important for our work, we now explain it in some detail.
Dislocations are defects in an atomic lattice, and they are central to the theory of plastic deformation. A dislocation can be viewed as a quantum of plastic slip: the smallest amount of plastic deformation that the lattice admits. Macroscopic, continuum-scale plastic deformation is the collective result of the motion of a large number of dislocations.
Models of plastic deformation vary depending on the scale at which they describe the system. At scales of millimeters or larger, plastic deformation is well described by continuum-level theories (see e.g. [14,Ch.6]). However, these continuum-level theories often break down at scales of 1-100 μm where the length scales of the specimen size and the dislocation distribution become comparable. At such smaller scales, a richer set of unknowns is used, the densities of dislocations, and equations are formulated for the evolution of these densities. At even smaller scales, the postulate of a 'smooth density' fails, and a description becomes necessary in terms of the individual dislocations and their motion: such systems are called discrete dislocation systems. This paper is concerned with the transition between the latter two types of models: from discrete dislocations to dislocation densities, as the number of dislocations becomes large. A popular evolution model for dislocation densities was derived by Groma and Balogh in [34,35] and later refined in [36,37]. It describes the evolution of the density of 'positive' and 'negative' straight and parallel edge dislocations, which are represented by 'positive' and 'negative' points in two dimensions. This model, and elaborations of it [38,39], have been used in the engineering community to predict dislocation density profiles with surprising accuracy [24,32,72,73]. The original system of equations from [35] is central to this paper; we will refer to it as the Groma-Balogh equations, and it appears in generalized form as equations (1.4) below.
The derivations in [34][35][36][37] are based on an upscaling argument starting from a system of discrete dislocations. None of these results are rigorous, however, since they build on uncontrolled approximations such as exchanging averaging with nonlinearity [35] or postulating a closure relation in the BBGKY hierarchy [34,39].
This brings us to the central question of this paper: can the Groma-Balogh equations be rigorously derived from an underlying discrete-dislocation system? We will see that the answer is subtle, and depends on how one decides to deal with the singularity of the interaction potential.

Formal Setup
The mathematical results of this paper are formulated for two different settings: a d-dimensional torus with isotropic evolution (where d = 1, 2 are the ones inspired by screw dislocations), and a two-dimensional torus with slip-plane confinement modelling edge dislocations. We describe these two situations and their physical interpretation in Section 2. At this stage, however, we illustrate the results just for the two-dimensional case with isotropic evolution. We work in a two-dimensional square torus T 2 , or equivalently a square in R 2 with periodic boundary conditions.
We model dislocations as points in T 2 ; they represent defects in a linearly elastic continuum medium. Systems of dislocations have an associated energy, which is the elastic energy of the stress and strain fields in the elastic medium, generated by the defects and by external loads. Formally, the quadratic nature of the continuum elastic energy leads to an expression of the form [18,50] Here x = (x 1 , . . . , x n ) ∈ (T 2 ) n and b = (b 1 , . . . , b n ) ∈ {−1, +1} n denote the position and the sign of each dislocation, U is a smooth external potential, and V (x − y) is a pairwise interaction potential which characterises the dependence of the elastic energy on the distance x − y between two dislocations. The potential V , which will be defined in Section 2, is related to the Green's function of the elasticity operator. Consequently, it has a logarithmic singularity at the origin with V (0) = +∞. The logarithmic singularity is central to this paper, and we will deal with it in detail in Section 1.3 below. We now describe the main question of the paper. Assuming that the velocities of the dislocations satisfy an isotropic linear drag law (Orowan's relation), their evolution in (T 2 ) n is of gradient-flow type, driven by the energy (1.1), namely dx dt (t) = −n∇Ẽ n (x(t); b). (1.2) By translating equation (1.2) into the language of measures, we find that the empirical measures of the positive and the negative dislocations, formally satisfy the aforementioned Groma-Balogh equations 1 ∂ t ρ + = div ρ + (∇V * (ρ + − ρ − ) + ∇U ) , (1.4a) This would suggest that as n → ∞, if μ ± n converge to limits ρ ± , then these limits should also be solutions of the same set of equations (1.4). The main aim of this paper is to investigate this convergence.
However, the formal arguments above cannot be made rigorous, because the singularity in V results in existence of solutions to (1.2) only up to the first time two particles of opposite sign collide. To resolve this blow-up, we replace (1.2) by a regularised version, which we introduce next.

Managing the Singularity
The singularity of V has its physical origin in the simplification of replacing the crystallographic lattice by a continuum linearly elastic medium and modelling the dislocations as point defects. These point defects generate stress and strain fields with infinite elastic energy in any neighbourhood of the defect. The energy of a single dislocation or of a finite set of dislocations-which in a genuine discrete model should be finite-is therefore infinite. 2 This infinite energy makes many energy-based methods unsuitable, and several approaches and alternative models have been developed to circumvent this difficulty: 1. the phase-field model developed by Peierls and Nabarro [31,44,49,51,53], 2. the removal of small balls around the dislocations from the elastic medium [18,30,50], 3. the smearing out of the dislocation core by a convolution kernel [4,13,20,30], 4. a cut-off radius within which dislocations do not interact [42]. 1 This well-known argument runs as follows: for a test function ϕ, we have The choice of the regularisation depends on factors such as: accuracy, computational convenience, the possibility to describe dynamics, well-posedness or the possibility to prove discrete-to-continuum convergence. In this paper we consider a broad class of regularisations that includes case (3) above: we replace the potential V by a smoothed, globally W 2,∞ potential V δ , where δ > 0 is a parameter with the interpretation of the length scale of the regularisation (see assumptions (V1)-(V4) in Section 2.2). In view of (1.4), we are interested in the limit δ → 0.
The regularised energy (denoted by E n without the tilde) is defined as (1.1), with V replaced by V δ and with the diagonal kept in the sum: Similarly to (1.2), the dynamics are now given by Note that since ∇V δ is globally Lipschitz continuous, this evolution is well-defined. By translating (1.6) into measures, we now find rigorously that the empirical measures μ ± n in (1.3), associated with a solution x of (1.6), satisfy the regularised Groma-Balogh equations in the weak sense. These equations are well-defined in the sense of distributions on (0, T )×T 2 whenever ρ ± are finite-mass measures (such as μ ± n ). Indeed, since ∇V δ is uniformly continuous on T 2 , so is the convolution ∇V δ * (ρ + −ρ − ), and therefore ρ ± ∇V δ * (ρ + − ρ − ) is a finite-mass vector-valued measure on T 2 for each t. This argument cannot be applied to the unregularised Groma-Balogh equations (1.4). There are, however, several ways to define a solution concept to these equations. We continue this discussion in §1.5.

Results of this Paper: Convergence and Non-convergence
We first describe our convergence result. When the regularisation δ is fixed, i.e., when we are dealing with a fixed, regular interaction kernel, the convergence of the discrete evolution equation (1.6) to the Groma-Balogh equations (1.7) as n → ∞ is standard; the technique goes back at least to Dobrushin [23]. Here, however, we will consider the joint limit n → ∞, δ n → 0, to which the standard theory does not apply.
Our main convergence result states that when δ n → 0 sufficiently slowly, convergence to the unregularised Groma-Balogh equations (1.4) holds. Theorem 3.3 specifies this result for the d-dimensional torus, and Theorem 3.9 specifies it for the two-dimensional torus with slip-plane confinement.
The meaning of 'how slowly' δ n needs to converge to zero for the result to hold depends both on the chosen time horizon T > 0, and on the sequence of discrete initial data for (1.6) approximating the initial datum of (1.4). Conversely, we also specify a lower bound on δ n such that our convergence result holds for a certain class of approximating initial data. In particular, if δ n 1/ √ log n, we recover the Groma-Balogh equations in the limit, under the assumption that n , which is natural in the case of a logarithmic singularity for the potential at zero. Note that in this regime the short-range interactions are governed by the model of the dislocation core, whose size is described by δ n ; the limiting Groma-Balogh equations, however, are independent of the description of the core.
Our second main result is a counterexample, showing non-convergence of the discrete evolutions to (1.4) when δ n → 0 fast enough, for a suitable choice of initial conditions. The key idea is to choose as discrete initial data a configuration of short dipoles whose mutual distance is infinitesimal as n → ∞, but much larger than the inter-dipole distance. In this case the discrete evolutions converge to limit measures ρ ± that are constant in space and time. This construction provides a counterexample to the discrete-to-continuum convergence whenever U is nonconstant, since in that case, on the torus, spatially-constant measures cannot be stationary solutions of the Groma-Balogh equations (1.4).

Comments and Perspectives
We comment on a number of aspects of this work and on some natural questions triggered by our results.
Conditions on the potential. The conditions (V1)-(V4) that we impose below on the interaction potential V cover many examples in materials science, such as vortices, Coulomb gases and dislocations. They are a mixture of fundamental conditions and conditions that we believe are mostly technical. The fundamental assumptions are the positivity of the Fourier transform, the singularity of V being at most logarithmic, and the convergence of the approximations. The logarithmic singularity of V is the strongest singularity under which the proof of the wellposedness of (1.4) in [15] (that we rely on in our proof) holds, and we are unaware of results that can deal with a singularity stronger than the logarithmic one. Positivity of the Fourier transform of the regularisation V δ of the potential V is needed in Lemma 2.5, where we establish a bound for the convolution with V δ that is crucial in the proof of the evolutionary convergence. Moreover, for regularised potentials V δ that do not have positive Fourier transform, the numerical simulations in van Meurs' thesis [67,Ch. 9] show that (1.6) can have a fundamentally different behaviour. Note that positivity of the Fourier transform also guarantees convexity of κ → V * κ dκ, which for κ = ρ + − ρ − is the interaction energy associated to (1.4).
Regularisation and a-priori estimates. There is a useful rule of thumb for the analysis of the properties of nonlinear PDEs, going back to the work of Jacques-Louis Lions and the French School of nonlinear PDE: 'if the right a-priori estimates can be established, then one can regularise any way one wants-without changing the results'. In other words, the equation determines the solutions, through the apriori estimates, and regularisations can only approximate such solutions. Even in cases where uniqueness is not obvious, such as the incompressible Navier-Stokes equations, this rule of thumb applies.
This rule-of-thumb requires, however, that the approximations do not violate the a-priori estimates. It is exactly this requirement that is not satisfied in this paper, and this is easy to recognize. The existence theorems, for slow δ n → 0 (Theorems 3.3 and 3.9) build upon the a-priori estimates first identified in [15]. These estimates are meaningful for solutions with bounded entropy, i.e., solutions ρ ± for which ρ + log ρ + and ρ − log ρ − are bounded. Empirical measures do not satisfy this condition, and therefore a 'regularisation' based on point measures, while physically meaningful, lies outside of this functional setting.
We nonetheless make use of the entropy-based estimates by using the fact that the regularised evolution has a bounded expansion rate in the Wasserstein metric, with a bound that deteriorates as δ n → 0. By constructing an intermediate object (i.e., the unique solution of the δ n -regularised Groma-Balogh equations (1.7) with a continuum initial datum, which is both entropically bounded and Wasserstein-close to the empirical measures), we can extend the entropic framework a little outside the finite-entropy realm. The price to pay is that the Wasserstein bound need not deteriorate too fast, and this translates into the slowness criterion of δ n → 0.
Beyond regularising the dislocation core. As an alternative to regularising the singular potential V , one can consider annihilation of dislocations, where dislocations of opposite signs are taken out of the system when they collide or are sufficiently close. This evolution is studied in [61,62] for finite n, in [6,9,41] on the continuum level, and in [66] a discrete-to-continuum convergence result is established. The main difference between the models listed above and the Groma-Balogh equations (1.4) is in the reversibility/irreversibility of the annihilation. In (1.4), if a positive and a negative dislocation meet, they form a short dipole, but if a sufficiently large force is applied to the system, they can break apart. In other words, annihilation is 'reversible'. In the other models, instead, annihilation is irreversible: once a short dipole forms, the two dislocations in it become permanently 'invisible' in the evolution.
Mixed-approach proof of convergence. Our proof of convergence is made in two steps, each requiring a different strategy. To estimate the distance between the empirical measures and the continuum solution of the δ n -regularised Groma-Balogh equations, we exploit the gradient-flow structure of the regularised equations of which they are both solutions (although with different initial data), and prove a Gronwall-type estimate in terms of Wasserstein distances. To estimate the distance between the intermediate measure and a solution of the unregularised Groma-Balogh equations we instead follow the approach in [15], based on entropy estimates.
Well-posedness for the Groma-Balogh equations (1.4). Various existence results for the Groma-Balogh equations have already been proved [15,26,27,46,48,70,71], and other related multiple-sign systems have been studied in [6,7,28]. A by-product of the convergence theorems in this paper provides additional existence results, which go beyond those cited above in allowing for more general interaction potentials.
The questions of uniqueness and stability appear to depend strongly on the regularity of the initial data. Mainini [48] proves uniqueness for a similar system in two dimensions with different boundary conditions, under the assumption that the solutions are in L ∞ , by using the log-Lipschitz continuity of ∇V * (ρ + − ρ − ). Li, Miao, and Xue [46] prove local-in-time uniqueness in H m ∩ L p , m > 2 and p ∈ (1, 2), and show that a finite existence time in these spaces implies blow-up in L ∞ .
Non-convergence. Our results fit into the setting of evolutionary convergence of multiple species interacting via singular potentials, e.g., [19], [67,Ch. 9], [65]. On the other hand, our counterexample shows that the discrete system does not always converge to the expected limiting equation, or worse, may not converge at all. In this paper we provide only a single counterexample, to prove the nonconvergence theorem, but the method of proof is very general: it relies on the fact that for fast δ n → 0 a short dipole is so strongly bound that it will not separate. The proof therefore can be adapted to prove a wide range of non-convergence results. Even more importantly, this strong binding will occur even if the initial data is not presented in already-bound form, since dislocations of opposite sign will quickly pair up into such short dipoles (see the simulations in [67,Ch. 9] for examples). Therefore we expect the non-convergence for fast δ n → 0 to hold for generic initial data.
This sparks questions for future research, such as: -is there an alternative notion of evolutionary convergence (e.g., statistical mechanics, convergence in probability on random initial data, addition of noise), weaker than the one in Theorem 3.3, for which convergence can be proven? -are there microscopic details invisible on the macroscale (such as the density of dipoles) which can affect the macroscopic behaviour, rendering the question of the discrete-to-continuum convergence much more subtle?
The organisation of the paper is as follows: in Section 2 we give a precise description of (1.6), (1.7) and (1.4) for both the isotropic and slip-plane confined evolutions, a detailed description of the assumptions and related properties of the interaction potential V and its regularisation V δ , and further preliminaries. In Section 3 we state and prove our main convergence results (Theorems 3.3 and 3.9). Our second main result, the class of counterexamples for convergence to the Groma-Balogh equations, is detailed in Section 4. Appendix A recalls the definitions and elementary properties of several Orlicz spaces.

Detailed Formulation of the Problems and Preliminary Results
Before describing the isotropic and anisotropic cases in detail, we first introduce the general setup in dimension d 1, and prove some preliminary results that apply to both cases.

Notation
signed and non-negative finite Borel measures on a generic set Ω; mP(Ω), m > 0 non-negative Borel measures of mass m on a generic set Ω (see also p. 8 for the notation P(T d × {±1})); Orlicz spaces on the flat torus (see Appendix A).

General Setup
We consider points x i ∈ T d with fixed signs b i ∈ {−1, +1} for i = 1, . . . , n that evolve according to (1.6). We assume the following conditions on the related potentials V , V δ , and U : . We refer to Appendix A for the definition of the Orlicz space Exp(T d ).
Remark 2.1. In the two-dimensional case, a possible choice for V is the Green's function on the flat torus T 2 . Its Fourier coefficients are given by A possible choice for its regularisation V δ is Given a point x = (x 1 , . . . , x n ) ∈ (T d ) n and the associated sign b = (b 1 , . . . , b n ) ∈ {±1} n , the discrete, regularised energy of the system is where δ > 0 (see also (1.5)). For what follows it is convenient to express the particle energy (2.1) in terms of the empirical measures associated to x and b.
We recall the definition of empirical measures (see (1.3)) Note that there is an obvious isomorphism between (x, b) and μ n , modulo relabelling the particles. Throughout the paper we will consider the pairs of measures μ = (μ + , μ − ) ∈ (M + (T d )) 2 such that μ + + μ − ∈ P(T d ). With a slight abuse of notation we will denote this class with P(T d × {±1}) (implicitly identifying the measure μ with a measure μ We define a continuum, δ-regularised energy E δ , that extends (2.1) to the whole space of probability measures P(T d × {±1}), as where, in analogy with (2.2), κ := μ + −μ − . Since the energy E n is invariant under relabelling the particles, We also recall the definition of entropy: for any With a little abuse of notation, here, and in what follows, we denote by ρ + (resp. ρ − ) a positive measure and its density with respect to the Lebesgue measure.
Finally we introduce the Wasserstein distance between measures in P(T d × {±1}). Let μ, ν ∈ P(T d × {±1}). We define the (square of the) 2-Wasserstein distance between μ and ν as and Γ (μ, ν) is the set of couplings of μ and ν, namely In the special case of μ ± (T d ) = ν ± (T d ), W enjoys some additional properties summarised in the next proposition.

Proof.
To prove (i), just note that the inequality W 2 μ, ν W 2 μ + , ν + + W 2 μ − , ν − is trivial, since the infimum in the definition of W is computed on a larger set. The opposite inequality follows by observing that it is more convenient to redistribute mass within T d × {1} and T d × {−1} rather than moving mass between the two, since diam(T d ) < 2. Property (ii) follows immediately from (i).
Next we extend [5,Theorem 8.4.7] to Wasserstein spaces on the torus. (2.7) Then, for every σ ∈ mP(T d ), it holds that Proof. Let 0 < t < T be fixed, let μ be a given solution of (2.7), and let h ∈ R be such that 0 < t + h < T . We prove that .6) with respect to x and y. The claim then follows by dividing (2.8) by h and letting h → 0, for both h > 0 and h < 0.
We now state an approximation result that will be used in the construction of approximate initial data for the evolution. For the definition of the Orlicz space L log L(T d ) we refer to Appendix A.

Lemma 2.4. (Approximation in W)
with nρ ± n (T d ) ∈ N and Ent(ρ n ) c, uniformly in n, such that

Proof.
We only give a sketch. We construct ρ n from ρ by moving mass of at most , the cost of this transport is at most The idea is to split T d into a d-cubic grid with cells of size of order n −1/d . Then, sequentially for each cell, we move at most 1/n mass to the next neighbouring cell such that each cell has mass with a value in 1 n N. For the so-constructedρ ± n , we construct μ ± n by placing in each of the cells nρ ± n (cell) particles (the precise location does not matter). An elementary computation yields that Finally, in the next result we prove a bound for the convolution with ∇V δ that will be crucial in establishing a priori bounds for solutions of the evolutionary problems.

Lemma 2.5. Let δ > 0, and let V δ : T d → R be a regularised potential satisfying conditions (V1) and (V2). Then there exists a constant c
, by the Parseval's Theorem and the Convolution Theorem we have where we have also used (V1) and (V2).
Remark 2.6. For slip-confined evolutions we will use the following anisotropic variant of (2.10), namely where ∂ 1 is shorthand for ∂ x 1 , which can be proved in the same way as (2.10).

Detailed Formulation of the Two Problems
In this section we describe the isotropic and anisotropic evolutionary problems separately.

Case 1: Isotropic Evolution in Dimension d 1 This is the case that we discussed in the introduction for
The difference between the isotropic case considered in this section and the anisotropic case of Section 2.3.2 is in the evolution. In the isotropic case the evolution equation is as introduced in (1.6), which in components and by (2.1) reads as In the two-dimensional case d = 2, this model is inspired by the study of the motion of straight and parallel dislocations, which can be represented by points in the plane. In particular, the evolution (2.11) (or (2.12)) is best compared to the evolution of screw dislocations, which are free to move in multiple directions. The isotropy assumption means that dislocations are allowed to move in every direction (see e.g. [3,10,11] for a more faithful treatment of preferred slip directions). When considered in the full space R 2 , screw dislocations generate an interaction potential V that is explicit: V (x) = − log |x| (up to material constants, which we disregard in this paper).
As the first step in establishing evolutionary convergence, we rewrite the evolutions of the particles in (2.11) in terms of the empirical measures μ ± n , defined as in (2.2), associated to their positions. This is convenient since the Groma-Balogh equations (1.4) that we want to obtain in the many-particle limit n → ∞ of (2.11) are given in terms of measures too. In fact, for any fixed δ > 0, the empirical measures μ ± n are solutions of the regularised Groma-Balogh equations The convergence result, Theorem 3.3, states that, for δ = δ n → 0 as n → ∞ sufficiently slowly, μ ± n converge to solutions of the unregularised version (2.14) Definition 3.2 below specifies the solution concept for equations (2.14).  [60]. In both cases the potential scales as − log |x| for small |x|. The positivity of the Fourier transform of the potential (b) follows by specialising the discussion on V wall below to the one-dimensional case.

Case 2: Two-Dimensional Domain, Slip-Plane-Confined Motion
The case of edge dislocations naturally leads us to consider the case of a two-dimensional domain where the dislocations are confined to fixed slip directions, which we take to be horizontal (i.e., parallel to the first coordinate axis in T 2 ). Edge dislocations generate a different interaction potential than screw dislocations. In the case of horizontal slip, the interaction potential in R 2 is see, e.g., (5)(6)(7)(8)(9)(10)(11)(12)(13)(14)(15)(16) in [42]. We construct the potential V on T 2 by carefully summing over Z 2 shifted copies of V edge first in the vertical and then in the horizontal direction. 3 In [67, App. A] it is shown that the pointwise limit is well-defined for all x ∈ R 2 , except at the singular points (0, k), k ∈ Z, of any shifted V edge , and that V wall is vertically 1-periodic with exponentially decaying tails in the horizontal direction. A straightforward computation shows that (V M ) M∈N converges uniformly in R 2 away from the singularities; since the singular behaviour at each singularity is given by a translated copy of V edge ∈ L 1 loc (R 2 ), we find that the convergence in (2.15) takes place in L 1 loc (R 2 ). Together with the exponential tails, we then find that the following limit is well-defined in L 1 loc (R 2 ): in particular, all finite sums satisfy (2.16) for ϕ ∈ D((−1, 1) 2 ), and then Therefore, using the periodicity of V , it is easy to see that and hence, for every k = 0, The anisotropic and regularised evolution satisfied by the dislocation positions is where the energy E n is as in (2.1), and the confined gradient of a function f : Ω ⊂ R 2n → R is defined in components, for i = 1, . . . , 2n, as Hence in (2.19) it is only the horizontal component of the positions that varies in time, namely The empirical measures μ ± n defined in (2.2) and associated to the solution of (2.19) satisfy the regularised and constrained Groma-Balogh equations (2.20) The convergence result, Theorem 3.9, states that, if δ = δ n tends to zero as n → ∞ sufficiently slowly, μ ± n converge to solutions of the corresponding unregularised version, namely (2.21)

Convergence Results
In this section we prove that the solutions of the discrete gradient-flow equations (2.11) (or (2.19)) associated to the regularised energy (1.5) converge to limit measures that solve equations (2.14) (or (2.21)) provided that δ n → 0 sufficiently slowly.
We consider the two cases outlined in Section 2.3: isotropic in dimension d 1 and slip-confined in two dimensions. In both cases our approach builds on the existence proof given by Cannone, El Hajj, Monneau, and Ribaud in [15], where they introduce a functional framework in which the Groma-Balogh equations (2.21) for the slip-plane-confined case with U = 0 have a meaningful weak solution. The challenge they face is to give the nonlinear terms ρ ± ∂ 1 V * (ρ + − ρ − ) a meaning in the sense of distributions on (0, T ) × T 2 , for some T > 0: since ρ + and ρ − are a priori only measures, and ∂ 1 V is singular, this product need not have any meaning unless we make stronger assumptions on ρ ± . This is done by means of the following lemma, which has been proved in [15,Propositions 1.3] in the case d = 2, and is a key result in their analysis.
For the proof of this lemma for general d 1 we use part (iv) of Lemma A.1 and integrate in time. Then we conclude by the embedding of H In the next sections we describe and extend the functional framework of [15] for each of the two cases we consider, supplement it with new, quantitative discreteto-continuum estimates, and formulate and prove our convergence results.

Case 1: Isotropic Drag Law in Dimension d 1.
Here we consider the isotropic case introduced in Sections 1 and 2.3.1. We first discuss the different concepts of solutions that we use. For a regularised potential V δ the function ∇V δ * (ρ + − ρ − ) is smooth; therefore the equations (2.13) are a pair of convection-diffusion equations with smooth velocity fields. In particular the equations preserve the regularity of the initial data, and on finite time intervals no derivatives blow up. Therefore the concept of a solution poses no problems, and one can consider both smooth and measure-valued solutions of these equations. The empirical measures μ ± n constructed above from the discrete solutions of (2.11) are examples of such measure-valued solutions.
For the case of a singular potential V , we need to be more careful. We use Lemma 3.1 above to guarantee that the integrals involving ρ ± ∇V * (ρ + − ρ − ) are meaningful, and we define the concept of a solution as follows: The existence of a solution in the sense of Definition 3.2 will follow from our convergence Theorem 3.3 below. Uniqueness of solutions for such weak solutions is currently open; for stronger solution concepts, under assumptions of higher regularity, various uniqueness proofs have been constructed for related systems [27,46,48]. The main theorem of this section follows. We set λ δ := D 2 V δ L ∞ (T d ) and note that λ δ → ∞ as δ → 0, then we can state Let t → μ n (t) be the empirical measure of the solution t → x n (t) of (2.11) on [0, T ], with δ = δ n and initial datum μ •,n .
Then the limit ρ(t) := lim n→∞ μ n (t) exists (up to a t-independent subsequence) with respect to W, uniformly in t ∈ [0, T ], where ρ is a solution of the unregularised Groma-Balogh equations (2.14) in the sense of Definition 3.2 with initial datum ρ • . Remark 3.4. While (3.1) suggests that the choice of δ n depends on the initial data (μ •,n ), we can also reverse the dependence. Indeed, requiring instead that a class of approximating sequences (μ •,n ) n such that (3.1) holds for each such sequence.
Structure of the proof. We prove Theorem 3.3 by constructing an 'intermediate' trajectory ρ δ n : ρ δ n is obtained by solving the regularised equations (2.13) with the modified initial datum ρ •,n . We then show that W(ρ δ n , μ n ) vanishes as n tends to ∞ (as a consequence of Lemma 3.5) and that (ρ δ n ) converges to a solution of (2.14) (Theorem 3.6).
Proof. We split the proof into two steps.
Step 1: Existence. Let μ • ∈ P(T d × {±1}). The existence of a solution for the regularised equations (2.13) with initial datum μ • ∈ P(T d × {±1}) follows by discrete (in space) approximation. More precisely, from Lemma 2.4 we get is sequentially compact with respect to W (note that the domain T d is bounded, so the convergence in measure and in W are equivalent). Moreover, the map t → μ n (t) is Lipschitz continuous with respect to W, with Lipschitz constant independent of n (but depending on δ). To see this first note that, from the equations (2.13) satisfied by μ ± n we have that μ ± n (s)(T d ) = μ ± n (t)(T d ) for every s t, hence, by Proposition 2.2, it is sufficient to show that t → μ ± n (t) are Lipschitz continuous with respect to W . The latter follows, since, for every s t, we have that where we used (V4), and S n denotes the set of permutations of {1, . . . , n}.
By the refined version of the Ascoli-Arzelà Theorem we conclude that there exists a time-independent subsequence of (μ n ) (not relabelled) and a limit curve and We show that μ δ is a solution of (2.13) with initial datum μ • . First of all, μ n is a solution (in the sense of distributions) of (2.13) with initial datum μ •,n , namely Since, by construction W(μ •,n , μ • ) → 0, and since W(μ n (t), μ δ (t)) → 0 for every t ∈ [0, T ] by (3.3), we can immediately pass to the limit in the first and last term of (3.4) (note that convergence in W implies weak * -convergence of the positive and negative components). For the nonlinear term, we pass to the limit pointwise in t ∈ (0, T ), and conclude afterwards by applying the Dominated Convergence Theorem over the time integral. The spatial integral reads as Since (x, y) → ∇ϕ(x) · ∇V δ (x − y) is continuous on (T d ) 2 , we can directly pass to the limit n → ∞.
We now state the convergence of the regularised solution ρ δ , whose existence and uniqueness are established in Lemma 3.5, to a solution ρ of (2.14).

), and ρ is a solution of the Groma-Balogh equations (2.14) in the sense of Definition 3.2 with initial datum ρ • .
In what follows we use the shorthand L ∞ (L log L) for the space L ∞ (0, T ; L log L(T d )), and adopt this convention for any function space on (0, T ) × T d .

Proof. (Lemma 3.7)
We split the proof into two steps. In the first step we prove the claim for a further regularisation of ρ δ , obtained by means of a viscous approximation; we then deduce the claim for ρ δ in the limit for the viscous approximation parameter going to zero.
By differentiating in time the entropy of ρ ε,+ δ , and by using the (ε, δ)-regularised equations (3.10), we have, by (2.3), where κ ε δ = ρ ε,+ δ − ρ ε,− δ . Proceeding in the same way for the entropy of ρ ε,− δ , and adding up the resulting expressions, we have where in the last step we have used Lemma 2.5, which provides a constant c > 0 independent of δ and ε. By integrating the previous inequality over [0, t], for 0 t T , we finally conclude that namely ρ ε δ satisfies the claim (3.9).
We are now ready to prove Theorem 3.6, namely to connect the regularised solutions (ρ δ ) of (2.13), with initial approximate datum ρ •,δ , with a solution of the unregularised Groma-Balogh equations with initial datum ρ • .
We first note that ρ ± δ ∇V δ * κ δ is bounded in L 2 (L log 1/2 L). Indeed, by Lemma A.1 (v) and (vi) (integrated in time), and by (3.17), Using (3.19) and (3.17), we show that ∂ t ρ ± δ is bounded in L 2 (H −(d+1) ). Indeed, by Lemma A.1 (vi), and by using (2.13), we have that for any (H −(d+1) ). First, we note that by taking the difference of the equations (2.13) we have that ∂ i V δ * κ δ satisfies, for i = 1, . . . , d, in the sense of distributions, namely for any Using (3.19), we can then estimate the right-hand side of (3.21) in absolute value by which is uniformly bounded in δ by (V 2), since By applying Lemma A.2 with p = q = 2 to the triple vii)), we find that ∇V δ * κ δ is compact in L 2 (EXP), namely it converges strongly to f . Finally, we show that f = ∇V * κ. To see this, we compute the distributional limit of the sequence ∇V δ * κ δ . Let ψ ∈ C ∞ c ((0, T ) × T d ; R d ) be a test function; then we have By using (3.18) and assumption (V 3), we have for the last term that and by the uniqueness of the limit of ∇V δ * κ δ we deduce that f = ∇V * κ.
Step 3: The limit ρ ± is a solution of the unregularised Groma-Balogh equations. The solution ρ δ ∈ (L ∞ (L log L)) 2 of the regularised equation (2.13) with initial datum ρ •,δ satisfies the weak equations . We now show that, thanks to the compactness results in Steps 1 and 2, we can pass to the limit in (3.22) as δ → 0, hence showing that ρ is a solution of the unregularised Groma-Balogh equations, in the sense of Definition 3.2, with initial datum ρ • .
By (3.18), we can pass to the limit in the first and in the third terms of the first integral in equations (3.22). For the last term, the convergence is immediate, since ρ •,δ * ρ • as δ → 0. To pass to the limit in the nonlocal terms of equations (3.22), note that, by (3.18) and by Step 2, This concludes the proof of the theorem.
Finally, we prove our main result, Theorem 3.3, by combining Lemma 3.5 and Theorem 3.6.

Case 2: Two-Dimensional Domain, Slip Plane-Confined Evolution.
Here we consider the anisotropic case in two dimensions, as in Section 2.3.2. The main result of this section is Theorem 3.9, which is the analogue of Theorem 3.3 in this framework.
In analogy with Definition 3.2, we define the concept of solution for the unregularised and anisotropic evolution (2.21) as follows.
We set, as in the previous section, λ δ := D 2 V δ L ∞ (T 2 ) . The main theorem of this section is the following: Structure of the proof of Theorem 3.9. Again, we prove this theorem by constructing an intermediate solution ρ δ n of the regularised equations (2.20) with the modified initial condition ρ •,n with nρ ± •,n (T 2 ) ∈ N, and show that ρ δ n is close to μ n with respect to W, uniformly in time, and converges to a solution ρ of (2.21).
Proof. We split the proof into three steps.
Step 1: Existence, uniqueness and Gronwall estimate for (2.20) for fixed δ. The proof of the existence of a solution for (2.20) follows by discretisation via empirical measures, exactly as in Step 1 of the proof of Lemma 3.5. Similarly, the derivation of the Gronwall estimate can be done as in Step 2 of the proof of Lemma 3.5.
Step 2: Convergence of ρ δ to a solution ρ of (2.21). We split this step into two sub-steps: The derivation of a-priori bounds for ρ δ , in the spirit of Lemma 3.7, and the limit process as δ → 0.
Step 2.2: Convergence of ρ δ to a solution of (2.21). Here we can follow exactly the proof of Theorem 3.6 to deduce convergence of ρ δ to a solution ρ of (2.21), with respect to the weak * convergence in L ∞ (0, T ; (L log L(T 2 )) 2 ).
Step 3: Conclusion. Let (δ n ) be an infinitesimal sequence satisfying assumption (3.27). Let t → μ n (t) be the empirical measure of the solution t → x n (t) of (2.19) with initial datum μ •,n , and let ρ δ n ∈ C([0, T ]; P(T 2 × {±1})) ∩ (L ∞ (0, T ; (L log L(T 2 )) 2 ) be the solution of the regularised equation (2.13) with initial datum ρ •,n , whose existence and uniqueness are established in Step 1 of the proof, and whose bounds are proved in Step 2. Then, proceeding as in the proof of Theorem 3.3, we can extract a timeindependent subsequence of n (not relabelled) along which we have simultaneously

Non-convergence: A Uniform Distribution of Short Dipoles
In this section we construct counterexamples to the discrete-to-continuum convergence of gradient flows for the isotropic and the slip-confined cases of Section 2. More precisely, for the isotropic case in dimension d = 1, 2 and for the slip-confined case in dimension d = 2, we construct a family of initial data for the particle systems (1.6) such that the resulting discrete solutions do converge to a continuum limit, but this limit does not solve the corresponding Groma-Balogh equations (1.4). In Section 4.1 we explain the idea behind this construction, and heuristically describe how this choice leads to non-convergence. In Section 4.2 we state and prove the non-convergence result for the isotropic one-dimensional (Theorem 4.1) and two-dimensional cases (Theorem 4.4). Section 4.3 deals with the anisotropic case of edge dislocations.

Choice of the Initial Conditions
The strategy of the counterexamples is as follows. We assume that the regularisation parameter δ n converges to zero sufficiently quickly, and we construct a sequence of initial data for which the resulting solutions of (1.6) are constant in time, at least approximately. The continuum limit of these solutions is then constant in time, and therefore is not a solution of the Groma-Balogh equations (1.4), unless ∇U ≡ 0.
In Figure 1 we sketch our initial condition (x n • , b n • ) in the case of edge dislocations in a two-dimensional domain. We choose to position n 2 dipoles of width of order δ n at a distance of order at least 1 √ n from one another, under the assumption that δ n 1 n (the precise assumption on the relation between δ n and n will be specified in each section).
The idea behind our choice for the initial condition is the following. Since V blows up logarithmically at 0, −V δ n has a deep well around 0 of width proportional to δ n . We call a pair of a positive and a negative dislocation at (x n,+ •,i , x n,− •,i ) a short dipole if it 'fits' in this well (namely, if its width is smaller than the width of the well). By the logarithmic nature of the singularity of V δ n , the walls of this well are 1 δ n steep, so that it takes a large force to break this dipole apart.
On the other hand, the dipole-dipole interaction is weak: indeed the force field generated by a dipole at z n •,i is small at any y ∈ T 2 with |y − z n •,i | > c √ n , since the interaction forces ∇V δ n (x n,+ •,i − y) and −∇V δ n (x n,− •,i − y) generated by the positive and the negative dislocations in the dipole cancel out up to an error of order δ n . Similarly, also the net effect of the force −∇U generated by the external potential U on the dipole is of order δ n .
Hence, the evolution of the short dipoles governed by (1.6) is slow in time, and each dipole does not break apart. By choosing the initial positions carefully, and by making appropriate assumptions on the rate δ n → 0, we can then prove that the solution x n (t) of (1.6) is approximately stationary, namely x n (t) ≈ x n • for all t ∈ [0, T ], up to an error term that is infinitesimal as n → ∞.
The assumption that ρ + • = ρ − • is essential since it allows us to approximate ρ • with short dipoles (x n • , b n • ) as in Figure 1, with c = 1/ ρ + • ∞ . Then, the fact that the discrete solutions x n (t) of (1.6) with initial data (x n . However, if we assume that ∇U ≡ 0 on supp ρ • , then the limit stationary solution ρ • is not a solution to the limit equation (1.4).
In the remainder of this section we make the arguments above rigorous in the isotropic case in dimension one and two (Section 4.2), and in the two-dimensional slip-confined case (Section 4.3).

The Isotropic Case: d = 1 and d = 2.
Let T d be the d-dimensional flat torus, and let · T d denote the distance on T d defined in (2.6). Let δ n > 0 for every n ∈ N. We assume that V, V δ n , U : T d → R satisfy the following assumptions, in analogy with the ones listed in Section 2 (here the subscript I stands for 'isotropic'): ) there exist C, c > 0 , and a closed and simple C 1 -curve Γ n = ∂ B n , B n ⊂ B(0, Cδ n ) , such that max Γ n ∇V δ n · ν n −c/δ n for n large, where ν n is the outward pointing normal to Γ n ; The assumptions above are quite natural and are satisfied by the onedimensional model potential V δ n (s) = − 1 2 log(s 2 + δ 2 n ). Assumption (V 5) I mimics the bound (V 1) I on V , and forces the regularisation of the singularity to be localised in an interval around 0 with length asymptotically smaller than 1 n 1/d (which is the typical dipole-dipole distance in dimension d). Assumption (V 4) I provides an a priori bound on the force generated by a dislocation; this assumption can be easily relaxed by asking δ n ∇V δ n ∞ to be bounded for some ∈ N. Assumption (V 3) I identifies a force barrier of slope 1 δ n on the boundary of a region of diameter δ n , which needs to be overcome for a dipole to break apart. In dimension one the region of diameter δ n is an interval; in the two-dimensional case, this barrier lives on the boundary of a region B n contained in the ball B(0, Cδ n ) ⊂ T 2 , namely on a closed curve which encloses 0. Possible choices for Γ n are spheres of the form {s ∈ T 2 : s T 2 = γ δ n } or level sets of V δ n such as {s ∈ T 2 : V δ n (s) = −γ log δ n }. The precise choice of Γ n depends on the type of regularisation and on the symmetries of V .

The One-Dimensional Case
This is the case we describe in detail. The two-dimensional case will be briefly illustrated in Section 4.2.2, just by highlighting in what it differs from the one-dimensional setup treated here.
We consider a special arrangement of dislocations of alternated sign (− + − + . . . ) into short dipoles. This corresponds to the choice of n even and b i = (−1) i in the energy (1.5). It is convenient to re-label the positions of positive and negative dislocations as We now define a new set of variables (z, d) ∈ T n , for k = 1, . . . , n 2 , as follows: (4.1) The variable z k represents the position of the mid-point of the k-th dipole, while d k is the half-width of the k-th dipole. We consider the case of n/2 short dipoles, where the width of the dipole is much smaller than the dipole-dipole distance. This can be formally expressed by the condition max k |d k | min i = j |z i − z j | T . In terms of the variables (z, d) the energy (1.5) reads as and the gradient-flow equation (1.6) reads as d dt Relying on the evenness of V δ n , we rewrite the right-hand side of (4.2) as Hence, the discrete evolution of the short dipoles is described by the system for i = 1, . . . , n/2. We now introduce a subset of T n where we study the evolution; we will refer to it as the slow manifold. For any constant M > 0, we define the set Ω(M) ⊂ T n as where γ > 0 is defined in (V 2) 1 . ∈ Ω(2 A), the solution (z n (t), d n (t)) of (4.5)-(4.6) satisfies (z n (t), d n (t)) ∈ Ω(A) for every t ∈ [0, T ] and for large enough n. Moreover, the empirical measures μ ± n (t) and μ ± •,n associated to x n,± (t) and to x n,± • , respectively, where x n,± (t) and x n,± • are related to (z n (t), d n (t)) and (z n •,n 0 narrowly as n → ∞, uniformly in t ∈ [0, T ].
From here on, to ease the notation, we will drop the explicit dependence on n when it is clear from the context.

Proof.
The main idea of the proof is that the evolution of z is slow on the manifold, namely the forces n 2 ∂ z E n (z, d) acting on z are uniformly small. The forces on d may instead be large, but point in the 'right direction', i.e., there is a large basin of attraction to somed(t) which is close to 0.
The above argument will be made precise by means of three main steps. To this end, we define, for M > 0, In all our estimates the symbols C, c denote positive constants which only depend on U , V , A and the n-independent constants appearing in (V 2) I -(V 5) I .
Step 1: Behaviour of the gradient-flow equations (4.5)-(4.6) in Ω 2 (A). In this step we prove that the right-hand side of (4.5) satisfies the bound for all n large enough; (4.8) additionally, we rewrite the evolution of d i on Ω 2 (A) in a more convenient form.
To prove (4.8), we note that by the symmetry of V δ n the term = i in the first sum in the right-hand side of (4.5) is zero; for = i, we estimate the summand by using the Mean Value Theorem on the sum over q: 2n for all n large enough. By the assumption (V 5) I we then conclude from (4.9) that p,q=±1 For the forcing term (the second sum in the right-hand side of (4.5)), by (U ) we estimate This completes the proof of (4.8). Now we rewrite the evolution of the dipole width d i , under the assumption that (z, d) ∈ Ω 2 (A) during the evolution. We claim that, in (4.6), the term corresponding to = i is the dominant term. By isolating this term, we rewrite the evolution of d i as Step 2: The evolution (4.5) and (4.6) remains in the manifold Ω(A). We claim that the solution (z(t), d(t)) of (4.5) and (4.6) with initial condition for every t ∈ [0, T ], for large enough n. We first prove with a priori bounds that (z(t), d(t)) ∈ Ω 2 (A) for every t ∈ [0, δ 3 n ]. Then, we use Step 1 to improve these bounds and show that (z(t), d(t)) ∈ Ω(2 A − 2Cn 3 δ 4 n ) ⊂ Ω(A). In the final part we iterate this procedure in time to obtain the desired result on [0, T ].
Step 2.1: The evolution with initial data in Ω(B), B > A, stays in Ω 2 (A) for small time. We claim that the solution (z(t),d(t)) of (4.5) and (4.6) with initial condition , and for large enough n. By applying the bound (V 4) I for every term in the sum in the right-hand side of (4.3) and (4.4), we obtain the a priori estimate n∇ E n ∞ C/δ n for all n large enough.
Step 2.2: Improved estimates for (z(t),d(t)) for t ∈ [0, δ 3 n ]. Since (z(t),d(t)) ∈ Ω 2 (A) for every t ∈ [0, δ 3 n ], we obtain from (4.8) the improved estimate z(t) −z • ∞ Cn 2 δ n t Cn 2 δ 4 n , (4.11) which leads to x n,+ Then, we set x n,− • := x n,+ • . By construction, μ ± •,n ρ ± • as n → ∞, and z n • = x n,+ • and d n Note that (V 5 ) I is satisfied by our model example of V , so it reasonable to assume that it is satisfied by the regularised potential V δ n as well. In (4.9) we can interpret the sum over p and q as a four-point approximation scheme of the third derivative V  for all t ∈ [0, T ] and all n large enough, instead of (4.14), provided n 3/2 δ n → 0.

The Two-Dimensional Case
In this short section we only stress the differences with the one-dimensional case considered above. First of all, we introduce the subset of (T n ) 2 where we study the evolution, namely the slow manifold. In analogy with (4.7), for any constant M > 0, we define the set Ω(M) ⊂ (T 2 ) n as where B n is the region whose boundary is the 'trapping' curve Γ n in (V 3) I . The following theorem is the counterpart of Theorem 4.1 and Corollary 4.2 for d = 2: be a sequence such that n 2 δ n → 0 as n → ∞. Let U , V and V δ n satisfy conditions (V 1) I -(V 5) I and (U ) I , and let T > 0 be fixed. Let ρ • ∈ P(T 2 ) ∩ L ∞ (T 2 ), and let A • be the set of approximating sequences defined as and denote with μ ± n (t) the empirical measures associated to the solution x n (t) of (1.6) with initial datum (x n • , b n • ). Then, the weak limit of μ ± n (t), namely the measure is not a solution of (2.14) with initial datum Proof. The proof of Theorem 4.4 follows by a straightforward adaptation of the proof of Theorem 4.1 to the two-dimensional setting.
Note that the estimate (4.8) holds true, in the two-dimensional setting, with the bound Cnδ n (instead of Cn 2 δ n ), and this leads to the weaker condition n 2 δ n → 0 for δ n . Remark 4.5. (Sharper estimates under higher regularity) The extension discussed in Remark 4.3 has a two-dimensional equivalent. The bound on D 3 V δ n provides again an additional factor of δ n in the right-hand side of (4.8). To use the condition min i = j z i −z j T 2 c/ √ n, let us fix the index i, and relabel z such that z i −z T 2 is increasing in for = i. Since the balls B(z , c/(2 √ n)) are disjoint, for all R c/(2 √ n) the ball B(z i , R) contains at most Cn R 2 points z . In other words, there are at most Cn R 2 points z such that z i − z T 2 R. Hence, z i − z T 2 c √ /n for some c > 0. We use this estimate to replace (4.15) by Then, (4.8) becomes which leads to the weaker condition on δ n given by n 5/4 δ n → 0.
Given some δ n > 0, we define the slow manifold as The next theorem is the counterpart of Theorem 4.1 and Corollary 4.2 for a slip-confined evolution in dimension d = 2. Note that, unlike in Section 4.2, we do not consider a regularised potential V δ n , but we deal directly with V . where (z n • , d n • ) and μ ± •,n are defined in terms of (x n • , b n • ) via (4.1) and (2.2), respectively. Then A • = ∅. Now assume that ∂ 1 U ≡ 0 on supp ρ • . Let (x n • , b n • ) ∈ A • , and denote with μ ± n (t) the empirical measures associated to the solution x n (t) of the unregularised evolution (2.19), with initial datum (x n • , b n • ). Then, the weak limit of μ ± n (t), namely the measure ρ = (ρ + , ρ − ) such that μ ± n (t) ρ ± (t) as n → ∞ for a.e. t ∈ (0, T ), is not a solution of (2.21) with initial datum ρ • = (ρ • , ρ • ) in (0, T ). Proof. We start by establishing some properties of V that will enable us to proceed similarly as in the proof of Theorem 4.1.
Hence the extension of Theorem 4.1 follows similarly as in Section 4.2.2, with V δ n replaced by V . In particular, we note that the equivalent of the a priori estimates in Step 2.1 depends on r n . Hence, the time interval [0, δ 3 n ] may need to be shrunk when r n > 0 is small. Nevertheless, thanks to the r n -independently improved estimate in Step 2.2, the proof is easily adjusted to smaller time intervals. Remark 4.7. We note that with minor modifications to the proof it is possible to remove in Theorem 4.6 the lower bound on |d i · e 2 | in Ω(M) (i.e., to allow the two dislocations in a dipole to reside on the same slip plane) at the cost of introducing a regularisation V δ n similarly as in Section 4.2.2. Publisher's Note Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

A. Appendix: Orlicz Spaces and Embeddings
In this section we recall the definition and some properties of Orlicz spaces that we have used throughout the paper. This functional framework was used by [15] to prove existence results for the Groma-Balogh equations (2.21).
For brevity, we focus on real-valued Lebesgue-measurable functions on the flat torus T d , for any d 1. First we introduce Young functions (see [  It is easy to see that these Orlicz spaces are ordered, i.e., Exp α 2 (T d ) ⊆ Exp α 1 (T d ) for all 1 α 1 α 2 , and L log β 2 L(T d ) ⊆ L log β 1 L(T d ) for all 0 β 1 β 2 . For convenience, we set  . We will only be interested in the compact embedding of fractional Sobolev spaces into Orlicz spaces. For a more complete treatment of fractional Sobolev spaces we refer to [22]. (iv) there exists a constant C > 0 such that for all f ∈ L log L(T d ) and all g ∈ Exp(T d ); (v) there exists a constant C > 0 such that for all f ∈ L log L(T d ) and all g ∈ Exp 2 (T d );  [1,Thm. 8.16]. Property (iv) follows from [1,Thm. 8.11], since φ 1 (t) := e t − 1 and φ 1 (t) := t (log(e +t)) are complementary functions. To be precise, [1,Thm. 8.11] is valid for ψ 1 (t) := e t − t − 1 and ψ 1 (t) := (t + 1)(log(1 + t)) − t, which are complementary N -functions (unlike φ 1 and φ 1 ). In a bounded domain, however, since φ 1 , ψ 1 and φ 1 , ψ 1 have the same behaviour at infinity, the corresponding Orlicz spaces coincide, and the corresponding norms are equivalent. Finally we establish the compact embedding in (vii). First of all we recall that the natural embedding is compact for every 1 < α < 2 (this is true for every Ω ⊂ R d bounded, see e.g. [45]). We also recall that there exists an extension operator T : (Aubin-Lions-Simon) Let 1 p, q ∞ and X 0 , X, X 1 be Banach spaces such that X 0 ⊂⊂ X → X 1 . Then u ∈ L p (0, T ; X 0 ) : ∂ t u ∈ L q (0, T ; X 1 ) is relatively compact in L p (0, T ; X ) p < ∞, C([0, T ]; X ) p = ∞.