Variational analysis in one and two dimensions of a frustrated spin system: chirality transitions and magnetic anisotropic transitions

We study the energy of a ferromagnetic/antiferromagnetic frustrated spin system with values on two disjoint circumferences of the 3-dimensional unit sphere in a one-dimensional and two-dimensional domain. It consists on the sum of a term that depends on the nearest and next-to-nearest interactions and a penalizing term that counts the spin's magnetic anisotropy transitions. We analyze the asymptotic behaviour of the energy, that is when the system is close to the helimagnet/ferromagnet transition point as the number of particles diverges. In the one-dimensional setting we compute the $\Gamma$-limit of renormalizations of the energy at first and second order. As a result, it is shown how much energy the system spends for any magnetic anistropy transition and chirality transition. In the two-dimensional setting, by computing the $\Gamma$-limit of the renormalization of the energy at second order, we we prove the emergence and study the geometric rigidity of chirality transitions.


Introduction
Lattice systems are discrete variational models, whose energy depends on a spin field defined in a lattice.In frustrated lattice systems, spins cannot find an orientation that simultaneously minimizes the nearest-neighbor (NN) and the next-nearest-neighbor (NNN) interactions.Such interactions are said to be ferromagnetic or antiferromagnetic if they favour alignment or anti-alignment (we address the reader to [13] for a complete dissertation).
Three-dimensional frustrated magnets generally exist in the magnetic diamond and pyrochlore lattices (see [14]) and edge-sharing chains of cuprates provide a natural example of frustrated lattice systems (see [16]).Furthermore, jarosites are the prototype for a spin-frustrated magnetic structure, because these materials are composed exclusively of kagomé layers (see [20]).
A different frustration mechanism can also be caused by magnetic anisotropy, as it is common in spin ices (see [17]).Magnetic anisotropy refers to the dependence of the magnetization of a material on the direction of the applied magnetic field, which acts as a potential barrier (we address the reader to [23] for a comprehensive overview of magnetism, including a chapter on magnetic anisotropy and the energy barrier).The interplay between the two frustration mechanisms may result in very complicated Hamiltonians (see [22]).Most recently, the physics community attempts to find new fundamental effects such as the magnetization plateaus and the magnetization jumps which represent a genuine macroscopic quantum effect.For example, kagomé staircases have been of particular interest because of the concurrent presence of both highly frustrated lattice and strong quantum fluctuations (see [24]).
In this paper we study a frustrated lattice spin system whose spins take values on the unit sphere of R 3 .More precisely, a spin of the system u is a vectorial function whose codomain is the union of two fixed disjoint circles, S 1 and S 2 , of the unit sphere, which have the same radius R and are identified by two versors, v 1 and v 2 , Figure 1.We set the problem in one and two dimensions: in the one-dimensional case (Section 3) spin fields are parametrized over the points of the discrete set [0, 1] ∩ λ n Z and satisfy a periodic boundary condition; in the two-dimensional case (Section 4) they are parametrized over the points of the discrete set Ω ∩ λ n Z 2 , where Ω ⊂ R 2 is an open bounded regular domain.In both cases {λ n } n∈N is a vanishing sequence of lattice spacings.In the first setting, the energy of a given spin of the system u : where α ∈ (0, +∞) is the frustration parameter of the system that rules the NN and NNN interactions and {k n } n∈N is a divergent sequence of positive numbers.The term A(u) indicates the spins' magnetization direction (the so-called magnetic anisotropy) in the two circles.If the number of magnetic anisotropy transitions, i.e. the number of the jumps between the two circles, is finite, A(u) is a BV function and |DA(u)|(I) counts them.According to physical considerations, we require that the energy P n gives a penalizing contribution to the total energy.It is easy to see that while the first term of the energy E n is ferromagnetic and favors the alignment of neighboring spins, the second one, being antiferromagnetic, frustrates it as it favors antipodal nextto-nearest neighboring spins.A more refined analysis, contained in Proposition 3.5 and Remark 3.6, shows that, for n sufficiently large, the ground states of the system take values on one of the two circles and for α ≥ 4 are ferromagnetic (the spins are made up of aligned vectors), while for 0 < α ≤ 4 they are helimagnetic (the spins consists in rotating vectors with a constant angle ϕ = ± arccos(α/4)).The property of the latter case is known in literature as chirality simmetry: the two possible choices for the angle correspond to either clockwise or counterclockwise spin rotations, or in other words to a positive or a negative chirality.
In this paper, we address a system close to the ferromagnet/helimagnet transition point (see [15]), that is when α is close to 4 from below.We also require that λ n k n is close to some positive value (that can be also infinite).This assumption is reasonable, since from a physical point of view the change of the spin's polarization involves a larger amount of energy.Our aim is to provide a careful description of the admissible states and compute their associated energy.In particular, we find the correct scalings to detect the following two phenomena: the spins' magnetic anistropy transitions and chirality transitions that break the rigid simmetry of minimal configurations.
In [12], the authors studied a one-dimensional ferromagnetic/antiferromagnetic frustrated spin system with nearest and next-to-nearest interactions close to the helimagnet/ferromagnet transition point as the number of particles diverges.In that case, spin fields take values in the unit circle.The proposed model is different from that one, where no anisotropy functional P n was introduced.In [12] the presence of a periodic boundary condition allowed manipulating E n in such a way that it can be recast as a discrete version of a Modica-Mortola type energy, whose Γ-convergence is well-known in literature (see [18] and [19]).Indeed, expanding the functional at the first order, under a suitable scaling, spin fields can make a chirality transition on a scale of order approaches to a finite nonnegative value, as n → +∞ (otherwise no chirality transitions emerge).
To set up our problem, we let the ferromagnetic interaction parameter α depend on n and be close to 4 from below, that is, we substitute α by α n = 4(1 − δ n ) for some positive vanishing sequence {δ n } n∈N .As in [12], the Γ-limit of E n (with respect to the weak ⋆ convergence in L ∞ ) does not provide a detailed description of the phenomena (as a consequence of Theorem 3.12) and suggests that, in order to get further information on the ground states of the system, we need to consider higher order Γ-limits (see [6] and [7]).
The two phenomena can be detected at different orders.At the first order we are led to normalize the energy E n of the system and study the asymptotic behavior of (a rescaling of) the new functional Rescaling G n by λ n , we prove that magnetic anisotropy transitions can be captured when λ n k n is close to any positive finite value, for n large enough (see Theorem 3.16).At the scale value λ n , the energy spent for spin's magnetic anisotropy transitions is equal to the minimal energetic value corresponding to the sum of all the interactions in proximity of the transition points.In Figure 2 it can be seen an occurrence of the phenomenon that we are analyzing.Chirality transitions can be detected at the next order by means of a technical decomposition of the energy G n .The idea behind the construction in Subsection 3.6 is to split the problem set in the sphere into finitely many problems set in one of the two circles each.We associate each spin field u with a unique and finite partition of [0, 1] containing intervals I j such that u |I j takes values only in one circle.We note that the intervals I j depend on n because u is defined on the lattice [0, 1] ∩ λ n Z.We modify such restrictions u |I j in such a way that they still satisfy a similar periodic boundary condition on I j , denoting them as u I j .In Lemma 3.13 we decompose the functional G n as follows: The energy MM n is of discrete Modica-Mortola type and collects the pairwise interactions of spins' vectors pointing to the same circle; the functionals (R n ) j and (R n ) M(u) gather the interactions between consecutive spins' vectors that point to different circles.R n is a correction addend.The first sum and the other addend in the right-hand side of the previous formula need to be rescaled in different ways, the first sum being a higher order term.Thus, at the second order we deal with the energy In Theorem 3.18 we apply the Γ-convergence result contained in [12] to each functional MM n , rescaled by λ n δ 3/2 n .It turns out that different scenarios may occur, depending on the value of lim n λ n / √ δ n := l ∈ [0, +∞].If l = +∞, chirality transitions are forbidden.Otherwise a spin field can make a chirality transition on a lenght-scale λ n / √ δ n .In particular, if l > 0, it may have diffuse and regular macroscopic (on an order one scale) chirality transitions in each S j whose limit energy is finite on H 1 (I j ) (provided some boundary conditions are taken into account); if l = 0, chirality transitions on a mesoscopic scale are allowed.In this case, the continuum limit energy is finite on BV(I j ) and counts the number of jumps of the chirality of the spin field.
Systems defined in planar structures are much more difficult to study, due to the higher dimensional setting (see [1], [4], [5], [10], [11]).We address here the two-dimensional analogue of the frustrated spin chain studied in the first part of the paper.The energy of a given spin of the system u : We assume that the functional P n (•; Ω) is bounded.The number α > 0 is the frustration parameter of the system and {k n } n∈N is a divergent sequence of positive numbers.The term |DA(u)|(Ω) is related to magnetic anistropy transitions.In the two-dimensional setting, they occur on the edges of the lattice Ω ∩ λ n Z 2 and the natural number is an upper bound on the spins' transitions from a circle to the other in Ω.
Motivated by the variational analysis of the one-dimensional problem, we assume that the frustation parameter depend on n and is close to the helimagnet/ferromagnet transition point as the number of particles diverges, i.e. α n → 4 − .In view of detecting spins' chirality transitions, which cannot be captured by means of the Γ-limit of the energy at the zero order, we are interested in the functional defined by which is the two-dimensional analogue of G n , up to additive constants.In [10] the authors studied a similar frustrated spin chain whose spin fields take values in the unit circle of R 2 .In [10, Theorem 2.1] they proved the emergence of spins' chirality transitions by means of the Γ-convergence of the functional H n with respect to the local L 1 -convergence of two chirality parameters.
In view of applying their result in our setting, we employ an idea that recalls the construction carried out in the one-dimensional problem.We restrict every spin u to connected open sets C s that partition Ω in such a way that u |C s takes values only in one circle.In order to avoid more complicated notation, we do not impose boundary conditions on ∂Ω and we state the result by means of a local convergence.We note that the sets C s depend on n because u is defined on the lattice Ω ∩ λ n Z 2 .
We decompose where H n collects the interactions of spins' vectors pointing to the same circle and (R n ) C s gathers the interactions between spins' vectors that point to different circles.While in the one-dimensional setting the partition associated with a spin contains intervals, which guaranty the compactness results stated, in this case the sets C s could be very wild, as the spacing of the lattice shrinks.Therefore, we require as additional regularity condition for the components C s , that is the BVG regularity.Its definition can be found in [21] and is recalled in Definition 4.1.
With this regularity assumption, we can apply the Γ-convergence result proved in [9] to each addend of the functional as it is shown in Theorem 4.5, that is the main result of Section 4. It turns out that chirality transitions are possible and they can take place both in the vertical and horizontal slices of C s .

Basic notation
Given x ∈ R, we denote by ⌊x⌋ the integer part of x.For a set K we denote by co(K) the convex hull of K, by #K the number of its elements and χ K its characteristic function.We write v • w for the Euclidean scalar product of the vectors v, w ∈ R 3 and by S 2 the unit sphere of R 3 .For all v ∈ R 3 we denote by π v the Euclidean projection on v and by π v ⊥ the projection on the orthogonal complement of v.If A is a subset of the Euclidean space we denote by A its closure respect the Euclidean topology.We denote by C a generic constant that may vary from line to line in the same formula and between formulas.Relevant dependencies on parameters and special constants will be suitably emphasized using parentheses or subscripts.
If I ⊂ R is an interval and all w ∈ BV(I; R 3 ), we denote by Dw ∈ M b (I; R 3 ) the distributional differential of w, and by |Dw| ∈ M b (I) the total variation measure of Dw.We say that a sequence {u n } n∈N converges weakly ⋆ in BV(I; R 3 ) to a function u ∈ BV(I; R 3 ) if and only if (see [3,Definition 3.11 and Proposition 3.13]).We denote it by u n ⋆ ⇀ BV u.Fixing v 1 , v 2 ∈ S 2 and R ∈ (0, 1), we define the set It is easy to observe that the set S i is a circle centered in v i √ 1 − R 2 and it can be easily verified that the sets S 1 and S 2 are disjoint.Throughout the paper we assume that R ∈ (0, R Max ).
If S is an open set of R N and C is a collection of open subsets of S , we say that C is an open partition of S if C does not contain empty sets and Given two vectors w = (w 1 , w 2 ), w = (w 1 , w 2 ) of R 2 , we define the function χ[w, w] := sign(w 1 w 2 − w 2 w 1 ), with the convention that sign(0) = −1.

Further notation and definitions
We let I = (0, 1) and we consider a sequence {λ n } n∈N ⊂ R + that vanishes as n → +∞.It represents a sequence of spacings of the lattice I ∩ λ n Z.
We introduce the class of functions valued in S 1 ∪ S 2 which are piecewise constant on the edges of the lattice I ∩ λ n Z and satisfy a periodic boundary condition: We will identify a piecewise constant function u : I → S 1 ∪ S 2 with the function defined on the points of the lattice given by λ n i ∈ I ∩ λ n Z → u i := u(λ n i).Conversely, given values u i ∈ S 1 ∪ S 2 for There exists a natural projection map A : L ∞ (I; S 1 ∪ S 2 ) → L ∞ (I; {v 1 , v 2 }) defined as follows: For each spin u, the function A(u) indicates the spins' magnetization direction and its jumps correspond the the spins' magnetic anisotropy transitions.In general, A can be defined analogously on L ∞ (I; K 1 ∪ K 2 ), if K 1 and K 2 are two disjoint subsets of R 3 containing, respectively, S 1 and S 2 .In this case, we remark that if a spin field u ∈ L ∞ (I; The last two properties imply that this partition is unique.We observe that, if u ∈ L ∞ (I; S 1 ∪ S 2 ) and The following definition will be useful throughout the section.

Some properties of L ∞ functions with values in a compact set
In this subsection we recall some classical properties of the Lebesgue space L ∞ (I; K), where K ⊂ R 3 is a compact set.The statements and the proofs are fully analogous if the setting is a N-dimensional Euclidean space.
Proof.Since the set K is bounded then, up to a subsequence, there exists f ∈ L ∞ (I; R 3 ) such that f n ⋆ ⇀ f .Now we prove that f (t) ∈ co(K) for almost every t ∈ I.For every ξ co(K) there exist an affine function h ξ : R N → R and α < 0 such that

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By the weak ⋆ convergence of { f n } n∈N we have that for any measurable set Hence, by the arbitrariness of A, we obtain by formula (3.6) we obtain f (t) ∈ co(K), for a.e.t ∈ I.
Now we prove the second statement of the proposition.Let u ∈ L ∞ (I; co(K)).There exists a sequence {u n } n∈N ⊂ L ∞ (I; co(K)) such that u n = m j=1 a j χ I j , where a j ∈ co(K) and I j ⊂ I is an interval, for any j ∈ {1, . . ., m}, and u n converges to u in L 1 (I; R 3 ).Hence, u n ⋆ ⇀ u.Therefore, without loss of generality, we may prove the statement for u = a ∈ co(K).
We define the following function: ), Proof.Since the space L 1 (I; R 3 ) is separable, every bounded subset of L ∞ (I; R 3 ) is metrizable with respect to the weak ⋆ topology of L ∞ (I; R 3 ).Hence the set L ∞ (I; K) is metrizable.Therefore, by Proposition 3.2, we have that the set L ∞ (I; co(K)) is the weak ⋆ closure of the set L ∞ (I; K). □

A useful abstract result
In this subsection we cite an abstract Γ-convergence result proved in [2] that will be applied in Subsection 3.5.For this purpose, we introduce the following notation.Let K ⊂ R N be a compact set and for all ξ ∈ Z let f ξ : R 2N → R be a function such that

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For any n ∈ N we define the functional space With the notation already used, we denote the value of the function u in the interval λ n (i + [0, 1)) by u i for all λ n i ∈ I ∩ λ n Z.We introduce the sequence of functionals F n : L ∞ (I; R N ) → (−∞, +∞] defined as follows: where For any open and bounded set A ⊂ R and for every u : Z → R N , we define the discrete average of u in A as Theorem 3.4 (See [2]).Let { f ξ } ξ∈Z be a family of functions that satisfies H1, H2, H3.Then the sequence F n Γ-converges, as n → +∞, with respect to the weak ⋆ topology of L ∞ (I; R N ), to where f hom : R N → R is given by the following homogenization formula .

The energy model and its ground states
This subsection is devoted to the mathematical formulation of the model and the characterization of its ground states.
Let α > 0 be a fixed parameter and let {k n } n∈N ⊂R + be a divergent sequence of positive numbers.Denoting and in general if J = (a, b) ⊂ I we define We define the energy of the system as the sum of two addends.The first addend is a bulk scaled energy of a frustrated F-AF spin chain, E n : PC λ n → (−∞, +∞), having the following form: The second addend of the energy, P n : PC λ n → [0, +∞), is a term of confinement in S 1 ∪ S 2 and is defined as follows: where A is the function defined in formula (3.2).We consider the family of energies Furthermore, we define the functional Thus we gain a new expression for E n : Thanks to this decomposition, we characterize the ground states of E n .
Proposition 3.5 (Characterization of the ground states of E n ).Let 0 < α ≤ 4.Then, for n ∈ N sufficiently large, it holds Furthermore, a minimizer u n of E n over PC λ n takes values only in one circle S ℓ , with ℓ ∈ {1, 2}, and satisfies Proof.Let us postpone the proof of the following equality: after the next claim.We claim that, for n sufficiently large, if u ∈ PC λ n is a minimizer of E n , then u(I) ⊂ S 1 or u(I) ⊂ S 2 .We may assume that the open partition associated with u is {I 1 , I 2 }, i.e.M = 2, and u(I 1 ) ⊂ S 1 , u(I 2 ) ⊂ S 2 .The general case M ∈ N can be proved similarly.We have that where c and we observe that Therefore by the formula (3.10) we have that min In order to prove the claim we are left to show that, for n ∈ N sufficiently large, min which is equivalent to prove that where we used formula (3.9).Since #I n (I) − #I n (I 1 ) − #I n (I 2 ) ≤ 2, R ≤ 1 and α ≤ 4, we have that, for n sufficiently large, because k n → +∞.We have proved the validity of (3.12).Thus, combining (3.12) and (3.11), we get min We prove that min We fix ℓ ∈ {1, 2} and consider u ∈ PC λ n such that u(I) ⊂ S ℓ .By geometric and trigonometric identities we deduce that where πu i := π v ⊥ ℓ u i .Of course an analogous statement holds for u i • u i+2 .Thus where we have defined Now we are led to minimize E n .We find its minimum by following the same argument in [12].With an easy computation similar to the one in (3.7), we remark that where We fix ϕ ∈ − π 2 , π 2 so that cos ϕ = α 4 .We may assume for simplicity of notation that v ℓ = e n .Let so that πu i = (R cos(ϕi), R sin(ϕi), 0).By trigonometric identities, we have that Remarking that H n (u) = 0, we combine the previous identity with (3.14) to get that min The computation of the minimum follows from (3.13).Now we consider a minimizer u ∈ PC λ n of E n .For n sufficently large, it must hold that u(I) ⊂ S ℓ , for some ℓ ∈ {1, 2}, and thus implying that H n (u) = 0.It follows that Squaring the modulus of both sides in the previous equality, we infer Hence which concludes the proof.□ From now on we assume that n is sufficiently large to satisfy the thesis of the above proposition.
Remark 3.6.The case α > 4 is trivial and the ground states of E n are all ferromagnetic, i.e. u i = u, for all i ∈ I ∩ λ n Z and for some u ∈ S 1 ∪ S 2 .Indeed, denoting by E (α=4) n the energy of formula (3.8) for α = 4, we have that for all u ∈ PC λ n .By the above proposition, the energy E (α=4) n is minimized on ferromagnetic states, which trivially also holds true for the second term in the above sum.The minimal value of E n is min

Zero order Γ-convergence of E n
In this subsection we study the Γ-convergence of E n at the zero order.With a slight abuse of notation, we extend the energies E n , P n , E n and H n to the space L ∞ (I; co(S 1 ) ∪ co(S 2 )), setting their value as +∞ in L ∞ (I; co(S 1 ) ∪ co(S 2 )) \ PC λ n .With a slight abuse of notation, we extend the projection map A to the space L ∞ (I; co(S 1 ) ∪ co(S 2 )) by setting for u ∈ L ∞ (I; co(S 1 ) ∪ co(S 2 )).Furthermore we define For further details about the weak ⋆ topology of a BV space we address the reader to [3,Remark 3.12].
We prove the following proposition, which relies on the properties contained in Subsection 3.2 and will be useful in this subsection.Proof.By Proposition 3.2 it follows that, up to a subsequence, u n ). Thanks to (3.16), up to the extraction of a subsequence, M = M(u n ) is independent of n ∈ N. Up to subsequence, I n j → I j in the Hausdorff sense, for some intervals I j and for any j ∈ {1, . . ., M}.Note that some I j could be empty.Let us fix j ∈ {1, • • • , M}.For all ε > 0 there exists n 0 ∈ N such that We define the following two sets: One of the following three alternatives may occur: In the first case we have that u n ∈ L ∞ ((I j ) ε ; S 1 ) for all n ≥ n 0 , up to finitely many indices of the sequence.Thus, by Proposition 3.2, u n ⋆ ⇀ u ∈ L ∞ ((I j ) ε ; co(S 1 )) and hence, by the arbitrariness of ε > 0, we obtain that u ∈ L ∞ (I j ; co(S 1 )).The second case is fully analogous to the first case.If we repeat the above argument for all j ∈ {1, . .., M}, we deduce that u n ⋆ ⇀ u.Finally, we get the thesis by remarking that The third alternative leads to a contradiction.Indeed, if it holds true, we can find two subsequences {n (1)  k } k∈N and {n (2)  k } k∈N such that u n (1)   k On the other hand, applying again Proposition 3.2, we infer that u n ⋆ ⇀ u ∈ L ∞ (I; co(S 1 ∪ S 2 )).Then, by the uniqueness of the limit in the weak ⋆ topology, we infer that u 1 (t) = u 2 (t) = u(t) for almost every t ∈ (I j ) ε , which is a contradiction since co(S 1 ) ∩ co(S 2 ) = ∅.□ Firstly, we study the Γ-convergence of E n .The following theorem relies on a straightforward application of Theorem 3.4.
Theorem 3.10.The sequence E n Γ-converges to the functional with respect to the weak ⋆ topology of L ∞ (I; R 3 ), where f hom : co(S 1 ∪ S 2 ) → R is defined by Proof.The result immediately follows by applying Theorem 3.4 to where u, v ∈ K := S 1 ∪ S 2 , extended to +∞ outside K. □ Remark 3.11.The function f hom defined in (3.17) does not depend on the parameter λ n .Therefore, in the theorem above the Γ-limit does not depend on the choice of λ n .Furthermore, an analogous statement of Theorem 3.10 above can be obtained if the functional E n is defined only in L ∞ (I; S ℓ ) for some ℓ ∈ {1, 2} (see [12,Theorem 3.4]).Its Γ-limit has the same form and it is finite on L ∞ (I; co(S ℓ )).
The following theorem is the main result of this subsection.Theorem 3.12 (Zero order Γ-convergence of E n ).Assume that there exists lim n→+∞ λ n k n =: η ∈ (0, +∞].
Then the following Γ-convergence and compactness results hold true.
(i) If η ∈ (0, +∞), then E n Γ-converges to the functional with respect to the D-convergence of Definition 3.7, where f hom and D are defined in (3.17) and (3.15) respectively.Moreover if with respect to the weak ⋆ topology of L ∞ (I; R 3 ), where f hom is defined in (3.17).Moreover if then, up to a subsequence, u n ⋆ ⇀ u for some u ∈ L ∞ (I; co(S 1 ))∪L ∞ (I; co(S 2 )).
Proof.We first deal with case (i).We start by proving the compactness result.Let {u n } n∈N ⊂ L ∞ (I; co(S 1 ) ∪ co(S 2 )) be such that sup for some C > 0. Thus we have that ∈ N. By formula (3.8) and by the definition of A, we compute for some constant C = C(α) > 0, where the last inequality is obtained by observing that Hence, the sequence {u n } n∈N satisfies the hypotheses of Proposition 3.9 and so we deduce the existence

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We finally prove the limsup inequality.Let u ∈ L ∞ (I; co(S 1 ) ∪ co(S 2 )).We may assume that u ∈ D. Since A(u) ∈ BV(I; co(S 1 ) ∪ co(S 2 )), it is not restrictive to suppose that the number of jumps of u from one circle to the other is one, i.e. |DA(u)|(I) = |v 1 − v 2 |.Furthermore, by the same density argument exploited in Proposition 3.2 and the locality of the construction, we may assume that where a 1 ∈ co(S 1 ) and a 2 ∈ co(S 2 ).Let {v j n } n∈N ∈ L ∞ (I; S j ) be the recovery sequence for the constant function a j obtained by the Γ-convergence result in Remark 3.11 with 2λ n as the spacing of the lattice, i.e. v j n ⋆ ⇀ a j and We define we deduce that u n D → u.We compute We observe that 1 2λn as n → +∞.By formulae (3.22), (3.23), (3.24), we obtain that Let us prove the liminf inequality.Let Up to the extraction of a subsequence, we may assume that the previous lower limit is actually a limit.By compactness, we infer that u n ⋆ ⇀u ∈ L ∞ (I; co(S 1 )) ∪ L ∞ (I; co(S 2 )).Hence, by Theorem 3.10, we obtain lim inf We finally prove the limsup inequality.Let u ∈ L ∞ (I; co(S 1 )), the case u ∈ L ∞ (I; co(S 2 )) being fully analogous.The recovery sequence obtained from Remark 3.11, {u n } n∈N ⊂ L ∞ (I; S 1 ), satisfies the limsup inequality.□

First order Γ-convergence of E n
In this subsection and in the following one we study the system when it is close to the helimagnet/ferromagnet transition point as the number of particles diverges.In what follows we let α = α n and we assume that α n → 4 − , as n → +∞, and that n is sufficiently large so that Proposition 3.5 holds true.
Once again, with a slight abuse of notation, we extend the energies E n , P n and E n to the space L ∞ (I; R 3 ), setting their value as +∞ in L ∞ (I; R 3 ) \ PC λ n .Similarly, we extend A from L ∞ (I; co(S 1 ) ∪ co(S 2 )) to L ∞ (I; R 3 ).
The main result of this subsection, Theorem 3.16, concerns the phenomenon of magnetic anisotropy transitions.Having in mind Proposition 3.5 and (3.9), we define the functional At this point we need to introduce modified spin fields in order to understand better the asymptotic behaviour of the energy G n .Let u ∈ PC λ n and let C n (u) = {I j | j ∈ {1, . . ., M(u)}} be the open partition associated with u, with I j = (t j , t j+1 ), for j ∈ {1, . . ., M(u) − 1}, and I M(u) = (t M(u) , 1).We set t M(u)+1 := λ n 1 λ n .Since u is piecewise constant on the edges of the lattice [0, 1] ∩ λ n Z, we have that t 1 = 0 and t 2 , • • • , t M(u)+1 are multiples of λ n , so that t j λ n ∈ N, for any j ∈ {2, . . ., M(u) + 1}.We define the auxiliary spin u I j : and we set , where w j ∈ S 1 ∪ S 2 is a vector such that the following boundary condition is satisfied in I j : We prove the following decomposition lemma.
}} be the open partition associated with u.We have where, for all j ∈ {1, . . ., M(u)}, and, for all j ∈ {1, . . ., Proof.Remarking that we may write After adding and subtracting the terms u t j+1 λn −2 • w j , for any j ∈ {1, . . ., M(u)}, we interchange u t j+1 λn −2 • w j and u t j+1 λn in the first and the third sums, for any j ∈ {1, . . ., M(u)}, obtaining We conclude the proof by computing where we used □ Remark 3.14.In the decomposition (3.28) of G n (u) the functional MM n ( u I j ) represents the energy of the j-th modified spin field u I j , which is localized in one circle.The remainders for such modifications, (R n ) j (u) and (R n ) M(u) (u), consist of the interactions between spins with values in two neighboring intervals, I j and I j+1 .Furthermore, they contain an additional term linked to the boundary condition (3.27).The term R n (u) contains a corrective addend.
The next theorem shows that the correct scaling of the energy to capture spin fields' magnetic anisotropy transitions is λ n .To this end, for M ∈ N, we set Theorem 3.16 (First order Γ-convergence of E n ).Assume that there exists lim n→+∞ λ n k n =: η ∈ (0, +∞).
We prove (ii).At the second order we split the global functional on the 2-dimensional sphere into finitely many functionals localized in circles, where we repeat the analysis lead in [12].For each circle S ℓ we define a convenient order parameter.
Let u ∈ PC λ n .According to the notation introduced in Subsection 3.6, for j ∈ {1, . . ., M(u)} and i ∈ λ n − 1 , we consider the pair u i I j , u i+1 I j of vectors that take values in S ℓ , for some ℓ = ℓ j ∈ {1, 2}.We associate each pair with the corresponding oriented angle θ i I j ∈ [−π, π) with vertex in the center of the circle S ℓ given by We set We extend w(t) = w t j+1 λn −1 , so that w is well-defined in the whole interval I.Note that we can define a map T n by setting We point out that the intervals I j of the previous definition may be also empty.
The next theorem shows that the correct scaling of the energy to capture spin fields' chirality transitions is n .
Theorem 3.18 (Second order Γ-convergence of E n ).Assume that there exist lim |Dw| (I j ).
-If l ∈ (0, +∞), for all h = (w, A(u ) for all j ∈ {1, . . ., M(h)}, there exists {h n } n∈N ⊂ PC λ n such that h n θ −→ h, (3.31) holds true for some constant C > 0 and -If l = +∞, for all piecewise constant functions h : .31) holds true for some constant C > 0 and Proof.We prove the statement only in the case l = 0, the other cases being fully analogous.We start by proving (i).Let {h n } n∈N ⊂ L 1 (I; R × {v 1 , v 2 }) be such that (3.31) holds true for some constant C > 0. By formula and Remark 3.15, we infer that n C, for all j ∈ {1, . . ., M(h n )} and n ∈ N.
It is easy to see that, up to subsequences, M = M(h n ) is independent of n ∈ N and the interval (I j ) n → I j = (t j−1 , t j ), in the Hausdorff sense, for every j ∈ {1, . . ., M(h n )} (it may happen that I j = ∅, for some j).In the following computations we drop for simplicity the dependence on n writing I j in place of (I j ) n .
Reasoning as in Proposition 3.5, thanks to (3.29), we compute where we set π u i nI j := π v ⊥ ℓ u i nI j , with ℓ = ℓ j ∈ {1, 2} such that u i nI j ∈ S ℓ .By the definition of u i nI j and geometric and trigonometric identities, we observe that where, for simplicity of notation, we have dropped the dependence on n of the angles θ i I j .Taking into account the previous formulae, we gain

.32)
The proof can be carried out as in [12,Theorem 4.2].For reader's convenience we give here its sketch.By trigonometric identities, it holds Moreover, taking into account the boundary condition (3.27), we can find a vanishing sequence We insert the previous two formulae in (3.32) and compute that is the thesis.□

Analysis of the two-dimensional model
In this section we analyze the problem in the two-dimensional case.Therefore we need to introduce proper notation and new definitions.

Further notation and definitions
Let {λ n } n∈N ⊂ R + be a vanishing sequence of positive lattice spacings.Given i, j ∈ Z, we denote by Q λ n (i, j) := (λ n i, λ n j) + [0, λ n ) 2 the half-open square with left-bottom corner in (λ n i, λ n j).For a given set S , we introduce the class of spin fields with values in S which are piecewise constant on the squares of the lattice λ n Z 2 : We will identify a function u ∈ PC λ n (R 2 ; S ) with the function defined on the points of the lattice λ n Z 2 given by (i, j) → u i, j := u(λ n i, λ n j), for i, j ∈ Z. Conversely, given values u i, j ∈ S for i, j ∈ Z, we define u ∈ PC λ n (R 2 ; S ) by setting u(x) := u i, j , for x ∈ Q λ n (i, j).
Furthermore, we define the projection function In this paper we will make use of the notion of BVG regularity.BVG domains and BVG functions have been introduced in [21] (see also [9,Section 3]).A bounded connected open set Ω ⊂ R 2 is called a BVG domain if Ω can be described locally at its boundary as the epigraph of a BVG function with respect to a suitable choice of the axes, i.e., if for every x ∈ ∂Ω there exist a neighborhood U x ⊂ R 2 , a function ψ x ∈ BVG(R) and an isometry We remark that smooth domains and polygons are BVG domains and BVG domains are Lipschitz domains.
As in the one-dimensional case we observe that, if u ∈ PC λ n (R 2 ; S The last two properties imply that this partition is unique.We remark that the sets C s are squares or union of squares.In particular, (4.3) ensures that u maps two confining sets of the open partition in different circles, if their intersection contain edges of squares.
The following definition will be useful throughout the section.

The energy model
Our model is an energy on discrete spin fields defined on square lattices inside a given domain Ω ⊂ R 2 belonging to the following class: A 0 := {Ω ⊂ R 2 : Ω is a simply connected BVG domain}.
Similarly to the analysis at the first and second order in the one-dimensional case, we split the functional H n as follows: ), as it is the limit of BV functions.In order to show the L 1 loc -convergence, we fix A ⊂⊂ C s .Since dist(A, ∂C s ) > 0, there exists ε > 0 such that A ⊂⊂ (C s ) ε .We obtain: which vanishes as n → +∞, up to subsequences.This leads to the convergence (w n , z n ) → (w C s , z C s ) in L 1 loc (C s ; R 2 ).Finally, we prove that curl(w C s , z C s ) = 0 in D ′ (C s ; R 2 ).If ξ ∈ C ∞ c (C s ), then suppξ ⊂ (C s ) ε for some ε > 0 and so curl(w C s , z C s ), ξ = − □ Now we state the main theorem of this section.The regularity assumption on Ω and on the open partition of h in the statement ii) are required in order to apply [9, Theorem 2.1 iii)] locally.As explained in [9] a simply connected BVG domain guaranties an extension property for BVG functions, which is needed to construct a recovery sequence for h.On the contrary, the proof of the liminf inequality i) actually works without assuming this kind of regularity (see [9,Remark 2.2]).

Mathematics in Engineering
Volume x, Issue x, xxx-xxx.

Figure 1 .
Figure 1. S 1 and S 2 circles of anisotropy transitions.
finite number of times, i.e.A(u) ∈ BV(I; {v 1 , v 2 }) and so |DA(u)|(I) < +∞, the interval I can be partitioned in finitely many regions where the function u takes values only in one of the two sets K 1 and K 2 .In other words, there exist M(u) ∈ N and a collection of open intervals, {I j } j∈{1,...,M(u)} , such that 1 and the collection of open intervals {I j } j∈{1,...,M(u)} satisfies (3.3), (3.4) and (3.5).

a 1 , a 2 ∈Corollary 3 . 3 .
K and for some λ ∈ [0, 1].Then the sequence u n (t) := h(nt) converges to u in the weak ⋆ topology of L ∞ by Riemann-Lebesgue's lemma.□The closure of the set L ∞ (I; K) with respect to the weak ⋆ topology of L ∞ (I; R 3 ) is the set L ∞ (I; co(K)).

Definition 3 . 7 .Remark 3 . 8 .
)) : A(u) ∈ BV(I; co(S 1 ) ∪ co(S 2 )) = A −1 (BV(I; co(S 1 ) ∪ co(S 2 ))).(3.15)It is natural to extend Definition 3.1 to any spin field u ∈ D. The following notion of convergence will be used.Let {u n } n∈N ⊂ L ∞ (I; co(S 1 ) ∪ co(S 2 )) and u ∈ D. We say that u n D-converges to u (we write u n D → u) if and only if u n ⋆ ⇀ u in the weak ⋆ topology of L ∞ (I; R 3 ) and A(u n ) converges to A(u) weakly ⋆ in BV(I; {v 1 , v 2 }).We observe that the notion of convergence introduced in the previous definition is induced by the smallest topology on D containing the set A : A is an open set of the weak ⋆ topology of L ∞ (I; co(S 1 ) ∪ co(S 2 )) or A = A −1 (U), where U is an open set of the weak ⋆ topology of BV(I; co(S 1 ) ∪ co(S 2 )) .

Proposition 3 . 9 .
Let {u n } n∈N ⊂ L ∞ (I; S 1 ∪ S 2 ) be such that A(u n ) ∈ BV(I; {v 1 , v 2 }),for any n ∈ N, and let C n (u n ) = {I n j | j ∈ {1, . . ., M(u n )}} be the open partition associated with u n .We assume that sup n∈N M(u n ) < +∞.(3.16)Then there exists u ∈ D such that, up to subsequences, u n D →u.
of u ∈ D such that, up to a subsequence, u n D → u.Now we prove the liminf inequality.Let {u n } n∈N ⊂ L ∞ (I; co(S 1 ) ∪ co(S 2 )) be such that u n D → u ∈ D. It is not restrictive to assume that {u n } n∈N ⊂ PC λ n .By the liminf inequality of Theorem 3.10 we have lim inf n→+∞ E n (u n ) ≥ I f hom (u(t)) dt.(3.20)On the other hand, by the lower semicontinuity of the total variation respect the weak ⋆ convergence in BV(I; {v 1 , v 2 }), we have lim inf n→+∞ P n (u n ) = lim inf n→+∞ k n λ n |DA(u n )|(I) ≥ η|DA(u)|(I).(3.21) Hence by formulae (3.20) and (3.21) we obtain lim inf n→+∞ .26) Combining (3.25) and (3.26), we deduce the limsup inequality.Now we deal with case (ii).Firstly, we prove the compactness result.Let {u n } n∈N ⊂ L ∞ (I; co(S 1 ) ∪ co(S 2 )) be such that sup n∈N E n (u n ) < C, for some constant C > 0. Thus we have that {u n } n∈N ⊂ PC λ n .With the same compactness argument used in the previous case, we deduce the existence of u ∈ D such that u n D → u.In particular u n ⋆ ⇀ u.By the lower semicontinuity of the total variation respect the weak ⋆ convergence in BV(I; {v 1 , v 2 }), remarking that E n ≥ −C(α), for some positive constant C(α), we get

□ 3 . 7 .
Let v ∈ BV(I; {v 1 , v 2 }) and {u n } n∈N ⊂ PC λ n be such that A(u n ) ⋆ ⇀ BV v and (3.30) holds.By assumption, {|DA(u n )|(I)} n∈N is bounded.Let C n (u n ) = {(I j ) n | j ∈ {1, . . ., M(u n )}}be the open partition associated with u n .Up to subsequences, we may assume that M = M(u n ) is independent of n.By Lemma 3.13, Remark 3.15 and the definition of R M we havelim inf n→+∞ G n (u n ) λ n Therefore lim n→+∞ G n (u n ) λ n = R M .Second order Γ-convergence of E nWe let α = α n := 4(1 − δ n ), where {δ n } n∈N is a positive vanishing sequence.
and for all {h n } n∈N ⊂ PC λ n