Circling the square: deforming fractional D-branes in type II/Ωℛ\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathrm{\mathcal{R}} $$\end{document} orientifolds

We study complex structure deformations of special Lagrangian cycles associated to fractional D-branes at ℤ\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathbb{Z} $$\end{document}2 singularities in Type II/Ωℛ\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathrm{\mathcal{R}} $$\end{document} orientifold models. By means of solving hypersurface constraints, we show how to compute the volumes of the most simple D-brane configurations. These volumes are given as a function of the deformation parameters depending on the D-brane position relative to the smoothed out singularity. We observe which cycles keep the special Lagrangian property in various deformation scenarios and what orientifold involutions are allowed. As expected, the volume and thus the tree level value of the gauge coupling hardly change for D-branes not wrapping the exceptional cycle on the deformed singularity, whereas the volume of D-branes passing through the singularity depends on the deformation parameter by some power law.


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inherited from the underlying torus, but have different contributions from Z 2 fixed points. As a result, the tree-level gauge couplings are identical at the orbifold point, but one-loop corrections differ in general [20][21][22][23]. We expect the difference already to show up at leading order once deformations away from the singular orbifold locus are turned on. More concretely, the gauge couplings need to be computed from where Π a denotes the cycle wrapped by D6-brane a and Π a its orientifold image. For special Lagrangian (sLag) cycles the volume is given by the integral of the holomorphic three-form, but upon deformations some fractional cycles can loose the sLag property while staying Lag, such that For which cycles this applies depends on the one hand on the choice of background sixor four-torus of four-dimensional Type IIA/ΩR or six-dimensional Type IIB/ΩR models, namely untilted (rectangular) or tilted tori [24]. 2 On the other hand, any potential cancellation depends on the choice of exotic O6-plane in the case of T 6 /Z 2M ×Z 2 backgrounds with discrete torsion. These are exactly the phenomenologically most promising Type IIA/ΩR models, since they admit rigid three-cycles implying the absence of unwanted matter in the adjoint representation [5,12,13,15,16] as well as exponentially suppressed D-brane instanton generated couplings [30][31][32][33][34][35].
To our best knowledge, complex structure deformations of sLag n-cycles [36,37] on T 2n orbifolds have to date not been studied in the context of D-brane geometries and their implications for low-energy physics. An early discussion of the geometry of deformations of T 6 /Z 2 ×Z 2 with discrete torsion [38] was performed in [39]. By contrast, blow-ups by means of Kähler moduli of codimension (2n−4) singularities have been studied systematically, see e.g. [40][41][42] for a large class of Type IIB/ΩI orientifold compactifications with holomorphic involutions and [43] for a T 6 /Z 2 ×Z 2 model of Type IIA/ΩR without discrete torsion. In the context of heterotic orbifold 3 models the blow-up procedure has been studied extensively in the recent years [45][46][47].
This article is organised as follows: in section 2, we briefly review the relevant ingredients of sLag cycles for D-brane model building on T 4 /(Z 2N ×ΩR) and T 6 /(Z 2M ×Z 2 ×ΩR) orientifolds. We set the notation for the subsequent discussion of deformations and identify the relevant complex structure moduli within the closed string spectrum. Several examples for fractional D-branes passing through Z 2 singularities are given, and the expected difference in the value of the tree-level gauge coupling constant for fractional D-branes with identical bulk part after deformation is highlighted. Section 3 is devoted to the inspection of sLag deformations by the hypersurface formalism. Several examples of orbifold models with 'horizontal' and 'vertical' D-branes on square tori are discussed in detail, and additional technical complexities for deformations of a variety of more general D-brane JHEP07(2014)124 configurations are showcased. Section 4 contains our conclusions, and in appendix A we collect phenomenologically interesting examples of global models with fractional D-branes, which expose the need of going beyond the special configurations discussed in the bulk of the present article.
2 Special Lagrangian cycles on T 4 /Z 2N and T 6 /Z 2M × Z 2 orbifolds In this section, we briefly review the construction of sLag three-(two-)-cycles on toroidal orbifolds T 6 /Z 2M × Z 2 with discrete torsion (T 4 /Z 2N ), which are customarily used for intersecting D6(D7)-brane model building. Our focus lies on the cycles and moduli spaces of those orbifolds with known global particle physics models, and in section 3 deformations of the corresponding sLag cycles away from the singular orbifold point will be discussed.
Intersecting Dp-branes and Op-planes with p = 6 (7) arise in Type IIA (IIB) orientifold compactifications on Calabi-Yau manifolds CY 3 (CY 2 = K3) if an antiholomorphic involution R : z i → z i for i = 1, 2, 3 (i = 1, 2) is introduced such that R(Ω n ) = Ω n and R(J Kähler Dp-branes preserve the same supersymmetry and are said to satisfy the same calibration as the Op-planes if they satisfy the sLag conditions (2.1) for the same choice of holomorphic volume form Ω n , cf. [1,36,37] for an extended discussion. In the rest of this article, we say that a sLag cycle has calibration (Ω n ) or is calibrated w.r.t (Ω n ) if (2.1) holds, and analogously a cycle has calibration (Ω n ) if (2.1) holds with Ω n replaced by iΩ n . A cycle is called Lag if it satisfies only the first condition J Kähler 1,1 Lag = 0 without specifying a calibration.
Denoting the sLag cycle wrapped by N a identical Dp-branes a by Π a , its R-image by Π a and the sLag cycle of the Op-planes by Π Op , the global consistency or RR tadpole cancellation conditions can be cast in the following form, a N a (Π a + Π a ) + Q Op Π Op = 0 with Q Op = −4 p = 6 −8 p = 7 , (2.2) and the sLag condition on each cycle ensures the simultaneous vanising of all NS-NS tadpoles.
For Dp-brane model building purposes, it is necessary to be able to explicitly construct the sLags and compute their intersection numbers and volumes. This can in particular be done on orbifolds of the factorised six-torus T 6 = 3 k=1 T 2 (k) for Type IIA/ΩR orientifolds (T 4 = 2 k=1 T 2 (k) for Type IIB/ΩR), where a Dp-brane wraps a factorisable three-(two-)-cycle, k=1 (n k π 2k−1 + m k π 2k ) and Π bulk ≡ orbifold images 3)

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with the one-cycles (π 2k−1 , π 2k ) spanning the k th two-torus T 2 (k) (cf. figures 1 and 2) and the toroidal wrapping numbers n k , m k ∈ Z coprime. For T 6 (T 4 ), a basis of three-cycles (two-cycles) is provided by the products of one-cycles Π ijk := π i ⊗ π j ⊗ π k (Π ij := π i ⊗ π j ). To obtain a basis of bulk cycles of the orbifold T 6 /Z N × Z M (T 4 /Z N ), one has to sum over all orbifold images. Using the same notation, one gets the intersection numbers The sLag conditions for a given bulk cycle can be fully expressed in terms of the wrapping numbers (n k , m k ) and the complex structure parameters ρ k per two-torus T 2 (k) by using the integrated and normalised version of (2.1) (cf. e.g. [13]), (Z a ) = Vol(Π a ) Vol 6(4) > 0 and (Z a ) = 0 with Z a ≡ 1 Vol 6(4) Πa Ω n , (2.5) as explicitly listed below in section 2.1 and 2.2 for each individual orbifold under consideration. Besides from the sLag condition, for D6-branes the volume of the wrapped three-cycle also determines the value of the tree-level gauge coupling g Ga for the corresponding gauge group G a , 4π , (2.6) and c a = 1, 2, 4 for bulk and the two kinds of fractional cycles defined below in equation (2.7), respectively. While the formula with Vol(Π a ) = Vol(Π a ) has been used extensively on the six-torus and at the orbifold point (see e.g. [18,22,[48][49][50]), we will see in section 3 that this equality of orientifold image volumes is violated for fractional three-(two-)-cycles in the deformed phase.
In the presence of one or three Z 2 symmetries, the cycle can be fractional and stuck at Z 2 singularities, respectively. The form of Π Z 2 or Π Z (k) 2 is determined by the following sets of choices: 1. The even-& oddness of wrapping numbers (n k , m k ) ∈ {(even,odd), (odd,even), (odd,odd)} determines two possible sets (σ k = 0, 1), each of which contains two Z 2 fixed points of T 2 (k) that are traversed by the torus cycle without (σ k = 0) or with a displacement (σ k = 1) from the origin (cf. below for details).

For each Z
(k) 2 twisted sector, the overall sign of Π Z (k) 2 is given by the Z and leaving the two-torus T 2 (k) invariant for some permutation (ijk) of (123).
As an example, the exceptional part of a fractional two-cycle on the T 4 /Z 2 orbifold reads with e αβ an exceptional two-cycle at the Z 2 fixed point αβ on T 2 (1) × T 2 (2) , where the pair (α,α) of T 2 (1) is set by σ 1 = 0 : σ 1 = 1 : , and (β,β) of T 2 (2) analogously (cf. figure 1 for the fixed point labels). A factorisable fractional two-cycle on T 4 /Z 2N with given wrapping numbers (n k , m k ) k=1,2 is thus fully specified by 2 5 = 32 choices of (σ 1 , σ 2 ; τ 1 , τ 2 ; τ Z 2 ), and a factorisable fractional three-cycle on 2 ) k=1,2,3 . At the orbifold point, the sLag condition for a fractional cycle is fulfilled if the bulk part is sLag and the above combinatorics of adding exceptional cycles is respected.
The intersection numbers among bulk cycles are computed in equation (2.4), and fixed points under Z n along T 2 (i) × T 2 (j) support (n − 1) exceptional two-cycles with their intersection form given by minus the Cartan matrix of the Lie algebra A n−1 , (2.9) Details for some fractional D7-brane models on T 4 /Z 2N orientifolds are given in section 2.1 and appendix A.1. The exceptional contributions Π Z (k) 2 to three-cycles at Z (k) 2 fixed points arise as tensor products of exceptional two-cycles along T 4 (k) ≡ T 2 (i) × T 2 (j) with a toroidal one-cycle along T 2 (k) , summed over fixed point contributions and orbifold images, , one can infer that exceptional two-cycles, which arise from the blow-up of different Z n fixed points, are permuted depending on the background lattices, but the twist sector is preserved (also for n = 2 [1]), (2.11)

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Worldsheet parity of bosonic states In section 3, we consider (complex structure) deformations of codimension two-and three-singularities away from the singular orbifold limit, respectively, for these models.
Before discussing various orbifolds explicitly, let us briefly summarise the stringy origin of the Kähler and complex structure moduli which encode the blow-ups and deformations away from the singular orbifold point. The worldsheet parity Ω = ± of the massless bosonic field content of Type IIB and Type IIA string theory in ten dimensions is for convenience given in table 1. The six-and four-dimensional massless bosonic closed string spectra arise by dimensional reduction and integration over ΩR-even and ΩR-odd cycles as follows: the NS-NS sector of both Type IIB/ΩR on K3 and Type IIA/ΩR on CY 3 contains besides the dilaton φ and truncated metric G µν the volume moduli v i and their axionic partners b i , which belong to hyper and chiral multiplets in six and four dimensions, respectively, as listed in table 2. Here, Π n− i denotes a R-odd n-cycle, and Π n+ j a R-even n-cycle. The hyperkähler property of the K3 surface implies that for a fixed Ricci-flat metric there is an ambiguity in the definition of the complex structure, see e.g. [51]. More precisely, a complex structure is specified by the cohomology class of Ω 2 as below in equation (3.21), whose real and imaginary part span a two-plane in H 2 (K3, R). The Kähler form then spans a line in H 2 (K3, R) which is orthogonal to that two-plane. The metric, however, only depends on the three-plane spanned by the two-forms (Ω 2 ), (Ω 2 ) and J Kähler 1,1 . The remaining freedom to rotate these three two-forms within the three-plane determines if a smoothed out singularity is blown up (using a Kähler modulus v) or deformed (using a complex structure modulus z).
The RR sector of Type IIB/ΩR on K3 contains the truncation and splitting into selfdual and anti-self-dual part of the two-form  B a-s.d.,j µν originate from integrals over anti-self-dual two-forms of the (self-dual) RR-form C 4 . Here one has to use the fact that the hyperkähler geometry on K3 contains three self-dual and 19 anti-self-dual two-forms, cf. e.g. the review [51].
The RR sector in Type IIA/ΩR orientifolds contains the vectors and axionic partners of the complex structure moduli (cf. e.g. [13,52]), with the complex structures c k associated to the (h 21 + 1) ΩR-even three-cycles on CY 3 . In equation (3.27) of section 3.3 these moduli, which at the orbifold point can be explicitly constructed, are used in the topological expansion of the holomorphic three-form.

Two-cycles on T 4 /Z 2N
Exceptional three-cycles in phenomenologically appealing orbifold compactifications to four dimensions arise as tensor products of exceptional divisors on T 4 /Z 2N with toroidal onecycles along an additional two-torus T 2 . Deformations away from the singular orbifold point thus consist of deformations of Z 2 singularities on T 4 times the relevant toroidal onecycle on T 2 . It is instructive to first study the technique of deformations in six-dimensional T 4 /Z 2N models and discuss subtleties related to special background lattices and D-brane configurations there. We will in particular distinguish between untilted and tilted lattices and enhancements of gauge groups U(N a ) → USp(2N a ) in the T 4 /Z 2 context. In the associated appendix A.1, we briefly mention additional subtleties, e.g. the reduced number of independent deformations, related to orbifold image cycles under the Z 3 subgroup in the T 4 /Z 6 case.
2.1.1 T 4 /Z 2 with shift vector v = 1 2 (1, −1) The antiholomorphic involution R enforces each two-torus lattice to be oriented such that R acts crystallographically (cf. e.g. the reviews [18,19]), see figure 1 for our notation.   Any factorisable bulk two-cycle on T 4 /Z 2 can be expanded as (2.14) In the following, we use the abbreviationm a k ≡ m a k + b k n a k with b k = 0 for untilted and b k = 1 2 for tilted tori, respectively, and correspondinglyỸ a 1 = n a 1m a 2 (etc.). Denoting the complex structure modulus per two-torus , the bulk RR tadpole cancellation and bulk supersymmetry conditions for fractional D7-branes can be written as RR tadpole: a N aX SUSY: where in the notation of equation (2.5) the quantity Z a = 2 k=1   Table 3. of complex structure of the two-tori; this includes in particular the option of square tori (ρ 1 = ρ 2 = 1), on which we will perform explicit calculations of deformations away from the singular orbifold point in section 3.2. The resulting gauge group is U(16) a × U(16) b with (up to hermitian conjugation 16 b → 16 b ) unique massless matter field content for any choice (x ∈ {a, b}) of Z 2 eigenvalues (−1) τ Z 2 x , discrete displacements (σ x 1 , σ x 2 ) and discrete Wilson lines (τ x 1 , τ x 2 ), 2 × (120 a , 1) + 2 × (1, 120 b ) + (16 a , 16 b ). (2.16) As first geometrically interpreted in [1], by giving suitable vev s to the antisymmetric representations (120), the corresponding D7-branes and their orientifold images pairwise recombine into pure bulk D7-branes, which can then be moved away from the R and Z 2invariant loci. In this way, the gauge group is broken to USp(16) a × USp(16) b , or by splitting each of these bulk D7-brane stacks into two parallelly displaced ones, the gauge [54] is obtained. The models with tilted tori clearly differ from those with untilted tori as can be seen from the number of tensor multiplets in the closed string sector, n T = 1, 5, 7 for the aa, ab, bb lattice [1,24], respectively. The closed string spectrum furthermore contains n closed,U H = 4 hyper multiplets from the untwisted sector comprising the size-and shapemodulus of each two-torus as well as n closed,Z 2 H = 16, 12, 10 hyper multiplets on the aa, ab, bb lattice, respectively, from the Z 2 twisted sector containing the blow-up and deformation moduli. The number n closed,Z 2 H depends on the choice of tilted background lattices by the pairwise identification of Z 2 fixed points under the antiholomorphic involution R as detailed in figure 1.
The massless closed string spectrum of Type IIB/ΩR on T 4 /Z 2 can be explicitly computed following the technique described e.g. in chapter 15.2 of [55]. With the abbreviated
As an additional special feature of tilted tori, for D7-branes parallel to one of the O7-planes ΩR or ΩRZ 2 , orientifold invariant fractional two-cycles Π frac which requires that at least one two-torus is tilted and a discrete displacement and Wilson line occur simultaneously. This can e.g. be seen by truncating the orientifold invariance condition for T 6 /Z 2 × Z 2 with discrete torsion in [13] to T 4 /Z 2 . As an exemplary model with tilted tori we study the configuration in table 4 with four stacks of orientifold invariant D7-branes, two of which are parallel to the ΩR-invariant O7-plane and the other two to the ΩRZ 2 -invariant O7-plane. The twisted RR tadpoles are cancelled by choosing pairwise opposite Z 2 eigenvalues. Supersymmetry holds for any choice of toroidal complex structure ρ i . Thus the results for the square tori (at ρ i = 2 in the notation of figure 1) from section 3.2 apply. The gauge groups are due to the orientifold invariance enhanced to USp(4) satisfies the condition 0 = 273 − 29 n T + n V − n H of a vanishing gravitational anomaly as required for any globally consistent model in six dimensions. In this example, the volumes of a 1 = a 1 and a 2 = a 2 (b 1 = b 1 and b 2 = b 2 ) are identical at the singular orbifold point, but differ upon deformation of (some of) the ten independent Z 2 fixed points as shown in section 3. Since in four-dimensional models, the volumes are related to the gauge couplings by equation (2.6), the present observation constitutes the first indication that tree-level gauge couplings that were identical at the orbifold point for two generic fractional D-branes are expected to differ in magnitude upon deformations away from the singular locus.
For T 4 /Z 2N orbifold models with 2N > 2, the number of independent Z 2 fixed point deformations is further reduced by Z N identifications as detailed in appendix A.1 for T 4 /Z 6 . This reduction can again be seen as a toy example for the phenomenologically appealing but more complicated T 6 /Z 2M × Z 2 geometries and their complex structure deformations.

Three-cycles on
Factorisable T 6 /Z 2M × Z 2 orbifolds with discrete torsion and rigid D6-branes on sLag three-cycles play an important role in the search for phenomenologically appealing and fully computable Type II string theory vacua. The T 6 /Z 2 × Z 2 orbifold with h Z 2 21 = 48 possesses the maximal possible number of three-cycles, which for the T 6 /Z 6 × Z 2 and T 6 /Z 6 × Z 2 orbifolds are reduced to h Z 2 21 = 14 and 15, respectively, due to the additional related Z 3 subsymmetry as detailed in appendices A.2 and A.3.
A new feature of the T 6 /Z 2M × Z 2 orbifolds with discrete torsion compared to T 4 /Z 2N stems from the fact that worldsheet consistency requires one of the four O6-plane orbits to be 'exotic', i.e. (η ΩR , η ΩRZ (1) 2 , η ΩRZ (2) 2 , η ΩRZ (3) 2 ) = (−1, 1, 1, 1) with the underline denoting all possible permutations. As explained in detail e.g. in [5,13], the exceptional divisors in each Z (k) 2 twisted sector might pick up an additional minus sign η (k) ≡ η ΩR · η ΩRZ (k) 2 under the orientifold projection depending on the choice of exotic O6-plane. As an important consequence, orientifold invariant three-cycles also exist without invoking tilted tori as exemplified in section 2.2.1, and gauge couplings g −2 Ga ∼ Vol(Π a + Π a ) can depend on only one Z (k) 2 twisted sector as demonstrated in section 2.2.1 and an example of phenomenological interest in appendix A.3. We use here the full classification of orientifold invariant three-cycles for any choice of tilted or untilted factorisable tori that was given in [13].
with discrete torsion has the following Hodge numbers [39], and exceptional three-cycles are constructed as . The orientifold image cycles depend on the choice of untilted or tilted tori as well as exotic O6-plane as summarised in table 5. As in the T 4 /Z 2 case of section 2.1.1, for untilted tori all 48 deformations of codimension JHEP07(2014)124 Table 5. Orientifold images of exceptional three-cycles on the T 6 /Z 2 × Z 2 orbifold with discrete torsion on a factorisable six-torus. The R-images α β of the fixed points αβ depend on the tilt two singularities are independent and associated to ε However, differently from T 4 /Z 2N , the set of b 3 = 2(h 21 + 1) three-cycles can for any choice of tilted tori be split into a symplectic basis of (h 21 + 1) R-even and (h 21 + 1) R-odd three-cycles. Tilted tori thus do not reduce the number of independent complex structure deformations in four-dimensional models.
As an illustrative example to study the effect of complex structure deformations on the three-cycle volumes and corresponding gauge couplings, we focus here on untilted tori and a D6-brane a parallel to the ΩRZ 4 . (2.21) The orientifold image cycle a is given by 4 .

(2.22)
The discussion below is independent of the choice of displacement parameters ( σ), and for simplicity we have taken ( 0). Switching on σ a is orientifold invariant and has (up to permutation of two-tori) e.g. been used in the context of D2-brane O(1) instantons in [32]. Any other choice of exotic O6-plane implies Π rigid

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and such a stack for η ΩR = −1 has been used e.g. in [5] to support the U(4) gauge group of a global Pati-Salam model, see also [12] for a similar model. In the notation of equation (2.5), the calibration condition at the orbifold point is , and the massless states in the Z 2 twisted sector of Type IIA/ΩR on T 6 /Z 2M × Z 2 with discrete torsion are explicitly given by (2.24) in analogy to the T 4 /Z 2 twisted states in equation (2.17). The bosonic field content of one NS-NS scalar c k plus one R-R axionic scalar ξ k per Z 2 fixed point (αβ) is again in agreement with the general spectrum in table 2. Matter states in the other Z (k) 2 twisted sectors are obtained by permutation of two-torus indices and the corresponding entries in SO(8) weight states. Since we do not consider twisted sector states of other order in this article, we refer the interested reader to the full list of states in each twist sector of T 6 /Z 2M ×Z 2 ×ΩR in [13]. The reduced number of independent complex structure deformations due to some Z 2M symmetry with 2M > 2 is detailed in appendices A.2 and A.3, with the latter containing a global model exhibiting key features of the deformation dependences discussed above.

Deformations of orbifold singularities and hypersurface formalism
This section discusses the hypersurface formalism which we use to describe sLag cycles on the deformed orbifolds. We start by introducing sLag cycles on elliptic curves, i.e. two-tori, in section 3.1.1, and at deformed isolated (local) singularities in section 3.1.2. These results will be carried over to the global deformation geometries in section 3.2 for T 4 /Z 2 and in section 3.3 for T 6 /Z 2 × Z 2 with discrete torsion. There, we look at different deformation scenarios and analyze the structure of the sLag cycles that arises. In section 3.2.2, we numerically compute integrals of the holomorphic two-form over such cycles, depending on the deformation parameters. All computations in this section are performed for (untilted) square tori and the two basic choices of sLag cycles per two-torus. In section 3.4, we comment on the increase in computational complexity for generalizations required to analyze phenomenologically appealing global rigid D6-brane models.

Lagrangian lines on elliptic curves
Since the starting point for defining toroidal orbifolds is the torus, we start with the description of a two-torus as a hypersurface, namely an elliptic curve E in the complex weighted projective space P 2 112 . This space is spanned by homogeneous coordinates x, v, y which are subject to scalings (x, v, y) ∼ (λx, λv, λ 2 y). The elliptic curve is defined as the zero locus of the polynomial
To get a map from the ordinary definition of a torus to the elliptic curve, we will use the Weierstrass ℘-function. We define the torus as T 2 = C/Λ with a lattice Λ = ω 1 Z ⊕ ω 2 Z with complex structure τ := ω 2 /ω 1 ∈ R. Then the Weierstrass ℘-function is given by and fulfils the differential equation Thus, if we identify ℘(z) = x/v and ℘ (z) = y/v 2 , we get a bijective map from T 2 to E. The Klein invariant is then given by j(τ ) = g 3 2 /(g 3 2 − 27 g 2 3 ). Although g 2 and g 3 are fully determined on the lattice Λ, j(τ ) uniquely represents a choice of complex structure and is thus invariant under the modular group SL(2, Z). Note that the Z 2 reflection z → −z, which is a symmetry of every torus, translates to (x, v, y) → (x, v, −y).
Conditions for Lagrangian lines. We will describe Lagrangian lines as fixed sets under an antiholomorphic involution σ of the space in question. In this way, they can -besides cycles wrapped by D-branes -potentially represent orientifold planes in a given string compactification. In case of a two-torus, one can always rotate the lattice Λ such that this involution takes the form 5 σ : z → z. This involution is a symmetry of T 2 if the lattice is invariant, i.e. σΛσ = Λ, or if τ and τ are related by SL(2, Z). Now, since j(τ ) is meromorphic with real coefficients, this is the case precisely if j(τ ) = j(τ ) = j(τ ) or j(τ ) ∈ R. Then we can rotate the lattice such that g 2 and g 3 become real. We can distinguish between two cases: • Tori with 1 ≤ j(τ ) are the untilted (a-type) tori of figure 1 since the complex structure can be represented by τ ∈ iR. The zeros i lie on the real line, and we order them as 4 < 3 < 2 to be consistent with the convention of figure 1. At the boundary, we find the square torus (j = 1 or g 3 = 0) and the degenerate torus (j = ∞).
• Tori with 1 ≥ j(τ ) are the tilted (b-type) tori of figure 1 where τ ∈ iR + 1/2. Here, two zeros of F (x, v) are complex conjugate to each other, 4 = 3 =: implying that the third one is 2 = −2 ( ). This agrees with the convention e.g. in figure 2. The boundary cases are the same as for the untilted tori, where the square torus is rotated by π 4 . In addition, we find the hexagonal torus at j(τ ) = 0 (g 2 = 0) which has an extra Z 3 symmetry given by x → e 2πi/3 x.
On each two-torus, we can find Lagrangian lines for each set of winding numbers (n, m) which are relatively prime and through any point on the torus. In the language JHEP07(2014)124 of the homogeneous coordinates x, v, y, it is in general hard to write down an equation for them, so we focus on those Langrangian lines which are represented by antilinear (i.e. antiholomorphic and linear) maps σ of the form where A is a complex 2 × 2 matrix. In order to be a valid involution, the map must satisfy the two conditions Note that for each choice of A, we get two values of β which differ by addition of π. Furthermore, matrices A which differ by an overall complex phase correspond to the same Lagrangian line. For testing the sLag property, we need the holomorphic one-form, This tells us that for each matrix A, the two choices for β differ in their calibration. The last expression is given since we will often work in the coordinate chart v ≡ 1. It turns out that for each choice of g 2 and g 3 , a finite number of Lagrangian lines arises in this way.
The results are summarised in tables 6 and 7.

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Antilinearly realised Lagrangian lines per square two-torus Table 6. Classification of antilinearly realised Lagrangian lines on untilted and square tori. Note that the pairs of cycles III a/b as well as IV a/b are connected by the Z 2 symmetry on the orbifold, see section 3.2.1. The subscripts a and b are not related to the two types a and b of two-tori, see figure 1.

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Antilinearly realised Lagrangian lines per hexagonal two-torus Table 7. Classification of antilinearly realised Lagrangian lines on tilted tori. For hexagonal tori (g 2 = 0) as special cases one gets additional lines by the symmetry transformation x → e 2πi/3 x. For shortness we write = + i .

Lagrangians on local deformations
As a next step to finding sLags on deformed global geometries, we first look for them in local deformations. We start with the deformation of a C 2 /Z 2 singularity and then move on to C 3 /Z 2 × Z 2 . The construction of a C 2 /Z 2 singularity as a hypersurface proceeds as follows. If z 1 , z 2 are the coordinates with Z 2 acting as (z 1 , z 2 ) → (−z 1 , −z 2 ), we can form a basis of invariant monomials by x i = z 2 i (i = 1, 2) and y = z 1 z 2 . These coordinates obey one relation, so we find The singularity is now indicated by solutions to f = df = 0 which happens at the origin. Thus, the deformation is obtained by adding terms of lower order than in (3.6). Linear terms in y and x i can be absorbed by proper redefinitions so that we only add a constant term with complex parameter ε, For ε = 0, there are no solutions to f = df = 0; so (3.7) describes a smooth space. In case of the local resolution, we can choose ε ∈ R by rotations of the coordinates. In the case ε > 0 we look at the solutions of the antiholomorphic equation x 1 = x 2 which represents two real equations, i.e. its solutions are Lagrangian surfaces. Inserting the relation into (3.7) implies that y 2 ∈ iR. Choosing the branch y ∈ R, we end up with a cycle E + that fulfils the equation of a two-sphere whose size is controlled by ε, namely (y) 2 + |x 1 | 2 = ε. We define the holomorphic two-form such that it reproduces the familiar result in the singular JHEP07(2014)124 limit, Note the similarity of the form of Ω 2 with the holomorphic form in equation (3.5) on the elliptic curve. The imaginary part (Ω 2 ) vanishes on the cycle, so the cycle is in fact sLag.
Integrating (Ω 2 ) over the exceptional cycle at the origin, we find its volume to be equal to 2π √ ε, which differs from the naive guess 4πε. If, however, ε < 0, the resulting exceptional two-cycle is given by E − = {x 1 = −x 2 , y ∈ iR}, one finds that Ω 2 restricted to it becomes imaginary. Thus E − has a different calibration from E + , and in particular it is odd under the orientifold, to match the generalised Gimon-Polchinski model as displayed in table 3. To sum up, depending of whether the deformation is done in positive or negative direction in ε, the exceptional cycle is either even or odd under ΩR.
The step to the singularity of C 3 /Z 2 × Z 2 is straightforward at the level of the hypersurface description. But when one considers deformations and sLag cycles, new issues arise. As in the two-dimensional case, we start with coordinates z i , i = 1, 2, 3 of C 3 and form a basis of Z 2 × Z 2 invariant monomials by x i = z 2 i (i = 1, 2, 3) and y = z 1 z 2 z 3 . Since they obey one relation, we recover the local singularity as a hypersurface, Here the singular locus f = df = 0 consists of three singular lines {x i = x j = x k = 0 |i = j = k = i} which intersect at the origin. In order to deform these singularities, we again add terms of lower order, where terms linear in y and terms of the form x i x j can be absorbed by redefinitions. Thus, we are left with terms linear in x i and a constant term, which gives a total of four terms. However, as argued in [39], string theory only provides three deformation parameters, and a generic deformation will always leave a codimension three singularity which is a conifold. This will put one restriction on the four deformation parameters, and we find, One easily sees that the conifold singularity lies at x i = √ ε 1 ε 2 ε 3 /ε i . Note that the involution x i → x i not only requires ε i ∈ R, but also ε 1 ε 2 ε 3 > 0 since otherwise the constant term becomes imaginary. We first discuss the simpler case where just one of the fixed planes is deformed, e.g. ε 1 = 0 , ε 2 = ε 3 = 0. One can then factor out x 1 in (3.10) and recover the deformed C 2 /Z 2 singularity when x 1 = 0. For x 1 = 0, we find a singular line at x 2 x 3 = ε 1 which shows that the singular lines x 2 = 0 and x 3 = 0 have merged together. The Lagrangian three-cycles, that arise from the deformation, are a product of the Lagrangian two-cycle in the x 2 -x 3 plane and a one-cycle in the x 1 plane of the form x 1 = e iφ x 1 . Due to the non-compactness of C 3 /Z 2 × Z 2 , we find a whole family of Lagrangian cycles parametrised by the phase φ such that for given calibration, one of them is special Lagrangian.
The case of a generic deformation ε i = 0 ∀i is a bit more involved. By rotations we choose all ε i to be real and positive. We want to find an equation for a Lagrangian cycle JHEP07(2014)124 similar to the one described above for just one deformation. In the Z (1) 2 twisted sector, the proper antiholomorphic equations are ε 2 x 2 = ε 3 x 3 and x 1 = x 1 . Then (3.10) implies y 2 ∈ R, and we choose the branch y ∈ iR. With the additional assumption x 1 = 0 we can rewrite (3.10) as This describes a fibration of a two-sphere over the line x 1 ≥ ε 2 ε 3 /ε 1 with radius √ ε 1 − √ ε 2 ε 3 /x 1 . At the boundary x 1 = ε 2 ε 3 /ε 1 , the radius goes to zero, and the sphere degenerates to a point which closes the cycle. This point coincides with the conifold singularity found above. Furthermore, we define the holomorphic three-form such that it reproduces the familiar result in the singular limit, The three-cycle is sLag w.r.t. Ω 3 and is thus the exceptional cycle resulting from the deformation. Moreover, we can define other three-cycles analogously by permuting the homogeneous coordinates x i . Thus, in the generic deformed space, we find three exceptional sLag cycles associated to the Z (i) 2 (i = 1, 2, 3) twisted sectors, which intersect in the conifold singularity. However, the topological intersection number of these cycles is -in agreement with the orbifold language of section 2 -zero as can be seen by deforming the conifold. Analogously to the two-dimensional case, the sign of the deformation parameters ε i will determine the calibration of the exceptional three-cycle and thus its behaviour under the orientifold.

Global deformations as hypersurfaces
Finally, we can put the ingredients together to construct a hypersurface description of the global orbifolds that allow for deformations. We again start with T 4 /Z 2 : we take two elliptic curves as in section 3.1.1 with homogeneous coordinates y i , x i , v i , i = 1, 2 describing a T 4 . The Z 2 acts as (y 1 , y 2 ) → (−y 1 , −y 2 ) while leaving the other coordinates invariant. We thus define y = y 1 · y 2 as an invariant coordinate. In other words, we can consider this T 4 as a fibration of four points over P 1 × P 1 where the P 1 's are spanned by (x i , v i ) and the points are the solutions of the equation Then the Z 2 acts only in the fibre such that the quotient fibre is described by just one equation Instead of a complete intersection of hypersurfaces in a product of simple weighted projective spaces P 2 112 , we now have one hypersurface in a more general toric space [56,57] with weights q i given by the following table, The Calabi-Yau condition is fulfilled since the weight of the hypersurface polynomial f equals the sum of the weights of all coordinates. The singular locus (f = df = 0) is given

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by F 1 = F 2 = 0 and consists of 4 × 4 = 16 isolated points since each F i is of degree four. To find the generic deformation, we need to count all monomials of the same degree as f . The coefficient of the y 2 term is scaled to one. Terms linear in y are absorbed by shifting y accordingly to complete the square. The remaining terms are monomials of bidegree (4,4) in x 1 , v 1 and x 2 , v 2 . For each pair x i , v i we construct a basis of degree four monomials, which form a five-dimensional vector space. One basis element is F i (x i , v i ). We call the other basis elements δF where the index α = 1, . . . , 4 stands for the four fixed points per T 2 . The δF (α) i are chosen such that they have the same zeros as F i except for the α th one. For example we can choose, Now we can count the independent deformations. The coefficient of the F 1 F 2 term can be set to one by rescaling. Terms of the form F i · δF (α) j have four parameters, three of which can be absorbed by P GL(2, C) transformations on (x j , v j ). The remaining parameter represents the complex structure of the j th two-torus. We are left with 16 terms of the form δF , and we will see that each such term deforms exactly one singularity. To sum up, we give the explicit form of the hypersurface equation with the 16 deformation parameters explicitly, (3.14) The two more complex structure parameters of the tori are hidden in the expressions for F i (x i , v i ). We define the two-form on the global deformation space as More precisely, this definition describes a family of holomorphic two-forms, where the parameters can be seen in the precise expression for y from (3.14). The definition (3.15) reproduces the formula for the local deformation (3.8) in the limit v i → ∞ as well as the orbifold result in the singular limit ε a 1 ,a 2 → 0, where we use the product of one-forms on two elliptic curves (3.5) with the orbifold identification y = y 1 y 2 . Most of the time, we will work in coordinate patches of the form v i = 1 or x i = 1 where (3.15) simplifies accordingly. The construction of a deformable T 6 /Z 2 × Z 2 orbifold with discete torsion works analogously. One starts with three elliptic curves, parametrised by homogeneous coordinates x i ,v i ,y i (i = 1, 2, 3) and replaces the y i by the Z 2 ×Z 2 invariant y := y 1 y 2 y 3 which is subject to one constraint, (3.16)

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This equality describes a hypersurface in the toric space given by the weights q i as follows, The singular locus is F i = F j = 0 with x k , v k free for all (ijk) permutations of (123); it represents the 3 × 4 × 4 = 48 fixed lines of Z 2 × Z 2 , i.e. singularities of codimension two. These lines intersect in 64 codimension-three singularities at F 1 = F 2 = F 3 = 0. To go to generic deformations, we again classify the monomials which are allowed to modify f . As in the case with four compact dimensions, the important terms do not contain y. We distinguish between the following structures: • F 1 F 2 F 3 is the term whose coefficient is set to one.
k , with (ijk) a cyclic permutation of (123), give rise to the three complex structure moduli of the three two-tori after absorbing P GL(2, C) transformations in (x k , v k ). From the orbifold perspective in section 2, their coefficients are the untwisted moduli.
are 3×16 terms which correspond 1 : 1 to deformations of the (a j , a k ) singularity in the j −k plane. In the orbifold construction of section 2, the coefficients of these terms appear as twisted complex structure moduli.
• δF would give 64 additional deformation parameters. However, for given values of all other parameters, these are determined by the requirement that the whole space contains 64 conifold singularities, as for the local deformation. This follows again from the fact that string theory only provides moduli that deform the codimension two singularities, but not those of codimension three. The precise expressions for these parameters are in general not as simple as in (3.10).
To sum up, the equation for the space with generically deformed fixed planes is f = 0 with (3.17) with ε αβγ ε i αβ denoting the functions of ε i αβ , which ensure the existence of the 64 conifold singularities.
In section 2, we introduced three types of Lagrangian cycles on toroidal orbifolds, the bulk cycles Π bulk , the exceptional cycles Π Z 2 and fractional cycles Π frac . The fractional cycles are the most interesting ones because of their many discrete parameters. The questions that arise are, which of these cycles can be found in the hypersurface formalism for the resolution, and what are the restrictions on the parameters of the hypersurface equation.
To answer these questions we take the ansätze for the (s)Lag cycles from the elliptic curves For concreteness, we fix the complex structure of the two-tori to the square (i.e. ρ = 1 for untilted tori in the notation of section 2) which is done by setting g 3 = 0 in (3.1). Then by a rescaling, we choose g 2 = 4 such that the zeros of The advantages of the square torus are that it can be seen as either tilted or untilted (i.e. ρ = 2, 1 in the notation of figure 1), depending on how the lattice is embedded into C 2 . It therefore offers a bigger variety of Lagrangian lines defined by an antilinear involution than an arbitrary rectangular torus, see cases V to VIII in table 6.

sLags on the deformed T 4 /Z 2 on square tori
We start with sLag cycles on the deformation of T 4 /Z 2 , where we focus on cycles which appear in the T-dual of the Gimon-Polchinski model as described in section 2.1.1. Cycles which descend from sLag lines on the elliptic curves are already present at the orbifold point. Thus, we will first analyse them on the singular space and then check what happens when deformations are turned on. In order to specify a sLag cycle, we choose one antilinear involution for each pair of homogeneous torus coordinates x i , v i as in (3.4). This is always possible at the orbifold point if it is possible on the underlying two-tori. Therefore such sLags can appear as O7-planes. In this case, every deformation of the singularities must be compatible with the involution σ R . Those sLags on which D7-branes sit need a priori not to be fixed loci of antilinear involutions since the sLag condition is formulated using the Kähler form J Kähler 1,1 and the holomorphic two-form Ω 2 , see (2.1). This also holds for the exceptional cycles which need the deformation to have finite volume. Their local counterparts were introduced as fixed cycles of antilinear involutions in section 3.1.2.

Cycle structure
The first class of cycles corresponds to a product of Lag lines on the two two-tori. We denote them here as N 1 ⊗ N 2 where N i ∈ {I a , I b , II a , . . . , VIII}, cf. table 6. From the position of the lines in table 6, we can already conclude whether the corresponding two-cycle on the orbifold or its deformation will be a bulk cycle or a fractional cycle.
Cycles which do not pass through the Z 2 fixed points are representatives of bulk cycles. These are cycles which contain III or IV as one or two factors. 6 We can deduce their topology from their behaviour in the two complex x i planes. 7 • The cycles 8 III ⊗ III and IV ⊗ IV do not pass through the zero locus of y, and we can fix the branch cuts of the hypersurface equation (3.14) such that the cycles do not intersect the branch cuts. In this way, we see that each cycle consists in fact of 6 Although bulk cycles on the orbifold have moduli that allow them to change their position, the cycles III and IV are just the representatives at position (z) = 1/4, 3/4 or (z) = 1/4, 3/4, respectively, see   two disconnected components, which are distinguished by the sign of y. Since each factor is a circle in the x i plane, the whole cycle has the topology of a T 2 .
• If one of the factors is not III or IV, the projection of the cycle on the corresponding x i plane is a real curve whose endpoints are zeros of y. Thus, the two components y = ± √ F 1 · F 2 are glued together at these points and form an S 1 . Altogether these cycles are one copy of T 2 since the a and b components in the other factor (I i or II i ) have been identified.
Next we focus on cycles of type N 1 ⊗ N 2 with N i = I, II. If N 1 = N 2 , the cycle is, after choosing the proper sign, sLag with calibration (Ω 2 ), and otherwise the calibration is (Ω 2 ). Since these cycles fulfil (x 1 ) = (x 2 ) = 0, it is convenient to draw them in the real x 1 -x 2 plane. Note that the compactification of this plane is a T 2 since one needs to add circles at infinity to glue together the boundaries at x i = ±∞. The zero locus of y describes four horizontal and four vertical lines (at x i = 0, ±1, ∞) in the real x 1 -x 2 plane and divides it into 16 rectangles, where eight rectangles correspond to sLag cycles and the remaining eight are Lag but not sLag, see figure 3. In fact, each cycle consists of two identical rectangles differing only by the sign of y and glued together at the boundary (where y = 0), so the cycles look like a S 2 or more precisely like a T 2 /Z 2 . Therefore, they clearly represent fractional cycles as in equation (2.7). The parameters σ i ∈ {0, 1} are adjustable since each cycle exists either undisplaced (label a ⇔ σ i = 0) or displaced (label b ⇔ σ i = 1) from the origin, cf. table 6. This determines the choice of exceptional cycles JHEP07(2014)124 in equation (2.8), however their signs, encoded in τ Z 2 , τ 1 and τ 2 , are not clear as long as we are at the orbifold point. This issue will be resolved on the deformation in section 3.2.2.
We now turn to sLag cycles on the deformation space. These will on the one hand include deformations of the bulk and fractional cycles that we just encountered on the orbifold. On the other hand, we hope to see exceptional cycles that stem from the deformation itself and are shrunk to zero volume on the orbifold. For simplicity, we start with the deformation of just one Z 2 fixed point which will be at position (3, 3) on T 2 × T 2 since this corresponds to the origin in the x 1 -x 2 plane. 9 The hypersurface equation (3.14) with the expressions for F i , δF (α) i given in (3.13) and zeros of y at the Z 2 fixed points 2 = −1, 3 = 0 and 4 = +1 now becomes which confirms the fact that orientifolding removes half of the complex structure moduli. The effect of the deformation on the fixed locus of σ R is best visualised in the real x 1 -x 2 plane, where we find that two formerly separated zero-lines of y (x 1 = 0 and x 2 = 0) now combine into one zero-curve (namely x 1 x 2 = ε), see figure 4. If ε > 0, the cycles I b ⊗ I b and II b ⊗ II b start to shrink with growing ε. Although this by itself does not imply anything about the volume, we can already conclude that the Z 2 eigenvalue in (2.8) is negative, 10 (−1) τ Z 2 = −1, since at the point ε = 1 the cycle vanishes completely and thus its volume must decrease with the deformation. This fact tells us furthermore that the fractional cycle e 33 , which now has finite volume, has the same calibration as the bulk part Π 13 (or −Π 24 ) because both cycles are topologically components of the sLag cycle I b ⊗ I b (or II b ⊗ II b ). In section 3.2.2 we will confirm this quantitatively.
The cycles I b ⊗ II b and II b ⊗ I b on the other hand seem to have merged. This is necessary because the calibration of Π 14 (or Π 23 ) differs from the one of e 33 , and thus a fractional cycle of the form 1 2 (Π 14 ± e 33 ± . . .) (or 1 2 (Π 23 ± e 33 ± . . .)) cannot be sLag, cf. also the discussion of supersymmetry and combinatorics of fractional cycles in section 2. Instead, the newly created cycle must be the union of two fractional cycles, one with bulk part Π 14 and one with Π 23 , such that the exceptional part e 33 cancels out.
For the exceptional cycles we want to choose a similar ansatz as in the local case in section 3.1.2 with the involution σ : x 1 ↔ x 2 . Globally, however, this only works if we at the same time exchange the C * scalings and in particular the other homogeneous coordinates, σ : v 1 ↔ v 2 , y → ±y. For the fixed set of this involution we can rewrite (3.18), after a

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proper choice of branch, as   (y) (3.19) which still is the equation of a S 2 as long as |x 1 | < 1. This is ensured when we consider small deformations with ε < 1. This cycle is sLag with calibration (Ω 2 ) with Ω 2 as in (3.15), and its position in figure 4 is indicated by the dashed line. In case of a deformation with ε < 0, one finds a similar picture with an orientfold-odd cycle of calibration (Ω 3 ). This clearly explains why we observe fractional sLag cycle with bulk part Π 13 /2, but not with e.g. Π 14 /2: it has a different calibration from the exceptional part e 33 . One can engineer the fractional cycle Π 14 /2 by cutting the cycle The resulting boundary is a circle, and it divides the exceptional cycle into two hemispheres. Thus, we can take one such hemisphere to close the cycle, which will be of the form e.g. 1 2 (Π 14 ± e 33 ± . . .) where the ± in front of the deformed exceptional cycle e 33 comes from the ambiguity of which hemisphere is used. These fractional cycles have the same behaviour under the orientifold as required in the generalised T-dual to the Gimon-Polchinski model in table 3, namely (3.20) The whole discussion so far applied to the case of just one deformation in positive direction, ε 33 > 0. The exceptional cycle that appears is sLag with calibration (Ω 2 ), and the adjacent fractional cycles (I b ⊗ I b and II b ⊗ II b ) of same calibration and with negative exceptional contribution show up as sLag cycles made out of one component, whereas fractional cycles of different calibration had to merge to stay sLag. If we deform in negative direction, i.e. ε 33 < 0, we find the same picture just with switched roles. The exceptional cycle (in this case at x 1 = −x 2 ) is now calibrated w.r.t. (Ω 2 ), and we find that equally calibrated sLags (here I b ⊗ II b and II b ⊗ I b ) appear with negative exceptional part whereas the cycles I b ⊗ I b and II b ⊗ II b have merged together.
Since the deformation happens locally for small ε, this result applies to each singularity when we consider a general deformation. More precisely, each fixed point can be deformed in two directions such that the exceptional cycle becomes calibrated w.r.t. the real or imaginary part of Ω 2 . Before the deformation, there is a transversal crossing of the y = 0 locus with itself, indicating a singularity. Afterwards, the crossing point is (locally) replaced by two smooth non-intersecting curves, cf. the hyperbolas in figure 5. Switching on all deformations leads in general to a rather complicated cycle structure. As an example, in figure 5 we show the horizontal (I i ⊗ I j ) and vertical (II i ⊗ II j ) two-cycles, where all singularities are deformed such that the exceptional cycles have the same calibration. The corresponding cycles are listed in table 8. We see that all cycles with calibration (Ω 2 ) have merged to one connected sLag cycle (white area in figure 5), whereas those calibrated with (Ω 2 ) are fractional cycles with negative exceptional contribution.

Integrals of Ω 2 and numerical results
In the following part, we will compute integrals of the holomorphic two-form Ω 2 over the cycles that we just found on the deformed spaces. This is done as a function of the deformation parameters in order to show the dependence of these integrals on the deformation. The results will allow us to determine the cohomology classes of these cycles and in particular the exceptional parts of the fractional cycles.
Since we are integrating closed forms over closed cycles, the integrals are fully determined by the cohomology class of the two-form and the homology class of the cycle in question. More precisely, we expand the two-form class in a cohomology basis, such that the basis elements are Poincaré duals of integral cycles (indicated by square brackets in the equations below). For K3 as the deformed T 4 /Z 2 orbifold, such a basis is provided by the (Poincaré duals to the) six bulk cycles and the 16 exceptional ones, (3.21) Integrals are then expressed in terms of the topological intersection numbers given in equations (2.4) and (2.9). The complex structure is chosen such that z untw.
At the orbifold point, integrals of Ω 2 can be traced back to the product of two integrals of the holomorphic one-form Ω 1 defined in (3.5) over one-cycles on the elliptic curve. These  Figure 6. Integral of (Ω 2 ) over the exceptional cycle e 33 for a single deformation, depending on the deformation parameter ε 33 . Ω 2 is normalised to the value at the orbifold point. lead to elliptic integrals 11 K(k) which cannot be solved analytically. For example, we find for a horizontal cycle I a on the square torus We see that the integrals over all horizontal or vertical cycles have the same value, up to signs and factors of i, namely All integrals over sLag cycles on the deformed spaces are here evaluated numerically: we start with the case of just one deformation as in figure 4. Due to the symmetries x 1 ↔ x 2 and (x 1 , x 2 ) → (−x 1 , −x 2 ), we do not have to consider each cycle on its own but just a representative sample. The most interesting cycles are those which are directly related to the deformation, i.e. the exceptional cycles, and those fractional cycles which intersect the singularity, since they have contributions from the deformation modulus z tw. 33 . However, we also look at other cycles away from the deformed singularity in order to see if the parameter ε 33 plays a role there. In the following we will discuss the integrals on the various two-cycles.

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• Next we consider the integral over the cycle I b ⊗ I b (or equivalently II b ⊗ II b ) which is visualised by the solid curve in figure 7. For positive values of the deformation parameter, we see a non-analytic behaviour at the origin and an analytic computation shows indeed that which confirms that the cycle has a contribution −1/2 · e 33 , i.e. it is a fractional cycle with negative Z 2 eigenvalue.
• The other cycles of calibration (Ω 2 ), i.e. all other grey cycles in figure 4, turn out to give the same value for the integral, see the dashed curve in figure 7, although these cycles are not always related by symmetries in any obvious way. This follows from the fact that these cycles have the same bulk part, namely Π 13 /2 or −Π 24 /2, on the underlying square torus. However, the integrals are not constant but grow linearly with ε 33 , and we find z untw.
• Finally, we consider the integral of (Ω 2 ) over the cycles which are now as well calibrated by (Ω 2 ). The results are shown in figure 8. The integral on the merged cycle II b ⊗ I b + I b ⊗ II b (solid curve) turns out to be exactly twice the integral over each of the other cycles (dashed curve), which again are all equal. This result confirms that the merged cycle has no exceptional contribution and thus is the union of two fractional cycles with opposite Z 2 eigenvalue. Furthermore, we again observe a linear change, z untw. 14 = z untw.
To sum up, we have seen that the modulus z tw. 33 corresponds in lowest order to the square root of the deformation parameter ε 33 , whereas the untwisted moduli z untw. ij are also influenced by the deformation but in higher order, z untw. ij = const. + O(ε 33 ). Another result is that at ε 33 = 1, we obtain a new singularity and thus leave the geometric phase of a deformed orbifold singularity. This is indicated by the non-analytic behaviour of the integrals in figure 7 and the vanishing of the fractional cycle Finally, we discuss an example of a multiple deformation. We choose the deformation as shown in figure 5 with all singularities equally deformed, i.e. ε αβ ≡ ε for all α and β. Due to the shift symmetry on the underlying torus, all fractional cycles with calibration (Ω 2 ), i.e. the fractional cycles in table 8, lead to the same integral, which is plotted in figure 9. Qualitatively it shows the same behaviour as the integral for just one deformation in figure 7. In the series expansion around ε = 0, the factor of the √ ε term is four times  Figure 9. Integrals of (Ω 2 ) over fractional sLag cycles for a full deformation of all Z 2 fixed points, depending on the universal deformation parameter ε.
larger compared to the single deformation. This proves that the cycle under consideration is a fractional cycle whose four exceptional parts come with a minus sign as stated in table 8. Furthermore, the point where the integral becomes zero is exactly at ε = 1/16. This is not fully surprising since the true deformation modulus z corresponds, at least to lowest order, to the square root of ε divided by the before mentioned factor of four. The surprising point is rather that this factor four also holds for finite values of ε.
3.3 sLags on the deformed T 6 /Z 2 × Z 2 on square tori Since the main phenomenological interest lies in compactifications to four dimensions, we also discuss sLag cycles on the orbifold T 6 /Z 2 × Z 2 with discrete torsion and its deformations, in extension of the results of section 3.2. The orbifold perspective for this case was presented in section 2.2. We briefly analyze the structure of sLag cycles in this case and show the results for various types of deformations. For simplicity we choose the complex structure of the two-tori to be ρ = 1 in the notation of section 2, i.e. the tori are of square shape. The topological expansion of the holomorphic three-form reads However, only h 21 = 51, see equation (2.19), of the 104 parameters c are independent complex structure moduli: two of them can be absorbed by complex rescaling, and one half of the remaining parameters c are determined by the prepotential on the complex structure moduli space, see e.g. [59]. The orientifolding leads to 51 real complex structure parameters, cf. table 2.

Cycle structure
We start at the orbifold point, where we find bulk cycles and fractional cycles that descend from the underlying torus cycles in table 6. The most basic cycles to work with are again horizontal and vertical ones, and we focus here on cycles which pass through the fixed planes, i.e. cycles of the form N 1 ⊗N 2 ⊗N 3 with N i = I a/b , II a/b . Such a cycle is sLag with calibration (Ω 3 ) if the number of horizontal one-cycles in the factorisation (N i = I a/b ) is odd, whereas the cycle is sLag with calibration (Ω 3 ) if the number of horizontal cycles is even. These cycles lie in the real x 1 -x 2 -x 3 three-plane, and their boundaries are given by the zero locus of y in equation (3.16). This zero locus factorises into 3 × 4 two-planes at x i = −1, 0, 1, ∞, i = 1, 2, 3, in analogy to figure 3. In order to obtain exceptional cycles with finite volume, one has to switch on the corresponding complex structure deformations, which we will discuss step by step. The simplest class of deformations are those which deform only fixed planes from one twisted sector, e.g. ε 1 αβ = ε 2 αβ ≡ 0. 12 In this case every, three-cycle can be written as a product of a two-cycle on Def(T 4 (3) /Z 2 ), see section 3.2.1, and a one-cycle on T 2 (3) , see table 6, plus its image 13 under the remaining Z 2 . Accordingly, the holomorphic threeform factorises, Ω 3 = Ω 2 ∧ Ω 1 , as well as its integral over any three-cycle. This simple situation is suitable for describing the example of Vol(Π rigid a + Π rigid a ) for a rigid three-cycle perpendicular to the exotic O6-plane as in equation (2.23).
The discussion of a generic deformation turns out to be difficult because the functions ε αβγ ε i αβ , which are required to ensure that the full space contains 64 conifold singularities, cf. section 3.1.3, are hard to determine. However, we discuss two cases in which this is possible: • When we deform three fixed planes from three different sectors, which all intersect in one codimension three singularity, the hypersurface equation can be traced back to the equation for the local deformation (3.9).
• When all 3 × 16 fixed planes are deformed equally, we can use the symmetries that are preserved by that deformation, to find an expression for ε αβγ .

Deformation of three fixed planes
Here we choose the deformation of the three fixed planes that intersect at the fixed point (3,3,3) at z i = (1 + i)/2, with the same magnitude. For this we set ε 1 33 = ε 2 33 = ε 3 33 =: ε and find ε 333 = 2ε 3/2 , while the other parameters are zero. The hypersurface equation then simplifies to The fractional, horizontal or vertical, cycles then fall into three categories: 12 Observe that ε i αβ denotes the deformation parameter of the Z (i) 2 singularity through which the exceptional three-cycles ε (i) αβ ,ε (i) αβ pass. 13 In the hypersurface formalism, the orbifold image is automatically included.

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• There are cycles which do not intersect any of the deformed singularities. In the topological expansion of the integral of Ω 3 , they do not receive contributions from the twisted deformation modulus that we switch on, and thus we expect their volume to be constant to leading order with a subleading linear dependence on ε in analogy to figure 8. The fractional three-cycle Π rigid a I a ⊗ II a ⊗ II a in equation (2.21) is exactly of this type.
• For cycles, which intersect one of the singularities the discussion is similar to the T 4 /Z 2 case in section 3.2. For example, the cycle I a ⊗I b ⊗I b has the same calibration as ε • The cycles, which intersect all three singularities, are the most interesting ones. They are shown in table 9. The cycles which are products of only horizontal (group 1) or vertical (group 4) one-cycles have the same calibration as each of their exceptional components. Thus they constitute a fractional sLag cycle. The mixed cycles (groups 2 and 3) on the other hand contain exceptional contributions which are differently calibrated than the bulk part and thus cannot be fractional sLag cycles on their own. Instead, the three cycles in each group merge to one larger cycle such that the exceptional parts of wrong calibration cancel out. The resulting cycle is therefore sLag with calibration (Ω 3 ) for group 2 and calibration (Ω 3 ) for group 3. Accordingly, the zero locus of y splits into three branches, see figure 10. Note that the two branches that enframe the cycle from group 2 intersect at the conifold point The fractional cycle in equation (2.21) constitutes an explicit example of group 3 if one uses the shift symmetry on the underlying (T 2 ) 3 to replace the Z 2 fixed point locus (3,3,3) and corresponding deformation parameters by those at point (1,1,1).

Deformation of all fixed planes
Finally we discuss the deformation of all 48 fixed planes. To do so, we set all deformation parameters equal, i.e. ε i αβ ≡ ε for all i = 1, 2, 3, α, β = 1, . . . , 4. The hypersurface equation (3.17) then becomes We indeed find 64 conifold singularities at x i =x, i = 1, 2, 3 wherex is one of the solutions ofx 3 −x = ε(x 2 + 1) 2 . For small deformations, we observe the following horizontal and vertical sLag cycles:   • All purely vertical cycles (II a/b ⊗3 ) start to shrink, which indicates that they are fractional cycles whose exceptional part has negative sign, i.e. 1 4 Π 246 − i,αβε
• Cycles which are purely horizontal (I a/b ⊗3 ) also shrink, but not as fast as the vertical ones. This shows that they are fractional cycles also with negative exceptional contribution, schematically 1 αβ . In fact, they disappear at ε = 1/16. The discrepancy to the point where the purely vertical cycles disappear could be a signal that the exceptional cyclesε • The cycles with one vertical and two horizontal factors (II a/b ⊗ I a/b ⊗2 and permutations) have merged to one connected sLag cycle with calibration (Ω 3 ). One finds that this large cycle also shrinks and disappears at ε = 1/16 which can only be explained by negative exceptional contributions fromε αβ . The contributions from the cycles ε (i) αβ cancel out.
• All cycles with one horizontal and two vertical factors (I a/b ⊗ II a/b ⊗2 and permutations) such as the one in equation (2.21) have also merged in order to form one connected sLag cycle with calibration (Ω 3 ). However, it is not clear what sign their exceptional part has since at ε ≥ 1/16 they fill the whole real x i three-plane.
In addition, one observes that all but the purely vertical cycles intersect the conifold singularities.

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3.4 Towards more general D-brane configurations Tilted tori. The whole discussion of sections 3.2 and 3.3 was performed for orbifolds with underlying square tori. One advantage was that one could describe many horizontal and vertical sLag cycles in the real x i plane. However, many interesting orbifolds are based on tilted tori. The most simple example of T 4 /Z 2 with tilted tori in section 2.1 can be viewed as built on square tori rotated by e ±iπ/4 , with the consequence that the sLags can be constructed from products of the cycles VII and VIII (plus some exceptional cycles) in table 6. These consideration directly carry over to the T 6 /Z 4 orientifolds of [2]. Tilted tori are also of particular importance, if the orbifold group contains a factor of Z 3 , which also includes e.g. the Z ( ) 6 [3,4,[6][7][8][9][10][11]14] and Z ( ) [13,15,16,60] orientifolds of phenomenological interest. In case of a factorisable torus, each lattice must be the A 2 Lie lattice, which is a special case of a tilted torus. A computational challenge in discussing deformations lies the fact that two of the Z 2 fixed points are in the complex x plane, and the sLag lines, which intersect these fixed points, are described by circle equations, see table 7. Accordingly, the equations for these sLags become even more involved when switching on deformations.
Enhancing the orbifold group. The description of toroidal orbifolds as a complete intersection of hypersurfaces, which allows for a resolution of the singularities, is known for all factorisable orbifolds [58]. A description that allows for deformations is only known for Z 2 and Z 3 singularities in four compact dimensions and for Z 2 ×Z 2 and Z 3 ×Z 3 singularities in six compact dimensions. However, many interesting D-brane models are based on e.g. the Z 6 ×Z 2 [13,60] or the Z 6 ×Z 2 [13,15,16] orientifold. These orbifolds with D6-branes of phenomenological interest are chosen with discrete torsion, and some of their singularities can be deformed and give rise to three-cycles as discussed in appendices A.2 and A.3. One possibility to treat deformations on these orbifolds is to take the Z 2 × Z 2 subgroup discussed in the present article and mod out another Z 3 by hand. On the elliptic curve in equation (3.1), such an Z 3 acts by x → e 2πi/3 x. This will put some restrictions on the coefficients in the hypersurface equation, namely the elliptic curves must be shaped like the A 2 lattice (g 2 = 0), and Z 2 fixed points which are mapped onto each other under Z 3 must be equally deformed. Then the singularities in all Z 2 sectors can be deformed, but the fixed points of the higher order orbifold group elements stay singular. For the T 6 /Z 6 × Z 2 orbifold with discrete torsion, this ansatz could potentially be expanded by adding blow-ups of codimension two singularities in the Z 3 and Z 6 twisted sectors, cf. the discussion in appendix A.3. For T 6 /Z 6 × Z 2 with discrete torsion, however, no such clear separation of singularities exists, cf. appendix A.2.
Cycles with higher winding numbers (n, m). In this work we restricted to sLag cycles that were realised as fixed planes on antilinear involutions in the homogeneous coordinates. On the square torus, this gave us cycles with winding numbers (n, m) not exceeding ±1. Topologically, more general cycles can be constructed as sums of the horizontal and vertical ones, but this does not give us a sLag representative cycle. On the elliptic curve, one can draw these cycles in the complex x-plane and see their winding numbers in the JHEP07(2014)124 Note that due to the double cover structure, the cycle in the ℘ plane corresponds to a curve from −1 to ∞ which has the same winding behaviour as half the cycle in the z-plane.
winding around the points where y = 0. To compute integrals of the holomorphic volume form, one can choose a cycle with the same winding properties, which is easier to parametrise. Due to the closedness of the holomorphic volume form, the result is independent of the concrete cycle, but in general such a cycle will not have the sLag property. In particular, it is not clear if such a sLag representative also exists when deformations are switched on. One such cycle is shown in figure 11.
Choice of orientifold involution. In traditional orientifold models on toroidal orbifolds, the orientifold involution was chosen such that the O-planes topologically only contained bulk parts. However, here we have seen that, for the simplest antiholomorphic action on the homogeneous coordinates (σ : (x i , v i ) → (x i , v i )), one can obtain different sets of orientifold fixed planes. If σ : y → y and the deformation was such that ε > 0, the σ fixed set was the union of all purely horizontal and purely vertical fractional cycles of calibration (Ω), each with negative exceptional part , see e.g. figure 5. If, on the other hand, σ : y → −y (equivalently one could deform in ε < 0 direction), the fixed set is one large cycle which consists of all mixed horizontal-vertical cycles such that the exceptional parts cancel out. Thus, it seems that depending on the direction of the deformation we get either O-planes with or without exceptional part. In the orbifold CFT construction T-dual to the generalised Gimon-Polchinski model of section 2.1.1, one was required to use fractional cycles whose exceptional part gets a sign w.r.t the bulk part under ΩR which stay only Lag, but loose the sLag property under deformations, or in other words, such deformations would break N = 1 SUSY.
One can build models on the deformed smooth spaces in which the O-plane has exceptional contributions and where fractional cycles are sLag, and ask the question to what these would correspond in the orbifold limit.

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Furthermore, we have found involutions (x 1 , v 1 ) ↔ (x 2 , v 2 ) whose fixed set contains (integer multiples of) exceptional cycles. It would be interesting to see also in this case if such involutions have a correspondence of a fully fledged string theory compactification at the orbifold point.

Discussion and conclusions
In this article, we focussed on sLag cycles in type II orientifold models on T 4 /Z 2 and T 6 /Z 2 × Z 2 orbifolds. In particular, we were interested in the cycles when deforming the Z 2 fixed points or fixed planes. We used the formalism of describing these orbifolds as hypersurfaces in some toric variety, which allowed us to switch on deformations. Within this framework, a certain set of sLag cycles was described as fixed set under antiholomorphic involutions, which are potential candidates for orientifold symmetries. We saw how these symmetries set restrictons on the complex structure deformation parameters. Whereas at the orbifold point, one could only see the bulk part of a fractional cycle, on the deformation one could, depending on the deformation itself, identify the exceptional part. To this end, it was useful to explicitly compute integrals of the holomorphic volume form over these cycles. Furthermore, due to the sLag property, these integrals are equal to the volume of these cycles which in turn gives information about e.g. the tree level gauge coupling in the low-energy effective field theory. As expected, the value of the gauge coupling hardly changed for a D-brane away from the deformed singularity, whereas D-branes wrapped on the deformation locus showcased a power law dependence on the relevant modulus.
Another result is that certain sets of cycles had to merge with each other, because their fractional part had a different calibration from the bulk part. This would imply that such a deformation is only allowed if all cycles within such sets have the same number of D-branes wrapped around them. This is also visible when writing down the D-terms for the U(1) factors which descend from such D-branes.
One observation was that the more deformations are switched on, the more complicated are the precise descriptions of the cycles. E.g. the boundaries of the projection to the real plane become non-trivial to describe. Moreover, the observation in section 3.3.3 that threecycles parallel to the ΩR-invariant plane behave differently under deformation from those parallel to some ΩRZ (k) 2 -invariant plane seems to suggest that T-duality arguments used to permute all four kinds of O6-planes cannot be applied to deformed orbifolds.
As a next step, we plan to generalize this formalism to more general D-brane models, ideally to phenomenologically appealing ones. This will include orbifolds of tilted tori and orbifold groups of higher order as well as D-branes with more general winding numbers. In addition, the computation of integrals of the holomorphic volume form become highly involved on more general deformations, which is a problem that will be investigated in the future [61]. It will also be interesting to see if the discrete symmetries of [16,62] survive after deformation. Moreover, the deformations are also expected to affect the perturbative Yukawa couplings in models with fractional D6-branes [16,63,64] as well as the non-perturbative couplings generated by D2-brane instantons [30][31][32]35].

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Finally, the formalism of describing sLag cycles on deformed toroidal orbifolds is a priori a purely geometric construction which might also be applicable to other string / D-brane models.  Table 10. Consistent assignment of the reference point (upper entry) and the second Z (i) 2 fixed point (lower entry) contributing with sign factor +1 or (−1) τ a i to Π Z (j),j =i 2 a in dependence of the even-or oddness of the toroidal wrapping numbers, cf. [15] for details. support one exceptional divisor k per triplet of Z 2 fixed points e αβ with self-intersection number −2 per fixed αβ, where we have formally singled out e 11 from f (i) 11 as the exceptional divisor at the origin that is associated to the Z 2 twisted sector.

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As in the T 4 /Z 2 case, any fractional two-cycle on T 4 /Z 6 consists of a given bulk cycle with the combinatorics of assigning exceptional cycles in dependence of the evenor oddness of (n k , m k ) given in table 10 for convenience. The subtlety concerning the correct identification of the Z 2 twisted cycle in the origin can be avoided in D7-brane models by restricting to some non-vanishing displacement ( σ) = ( 0), but we refrain from discussing deformations of orbifold singularities at this point. The same reasoning holds for deformations of the T 6 /Z 6 × Z 2 orbifold in section A.2, whereas for T 6 /Z 6 × Z 2 there exists a clear geometrical separation of Z 2 singularities from Z 6 and Z 3 singularities as discussed in detail in appendix A.3.
To close the discussion of the T 4 /Z 6 orbifold, the counting of independent deformations or blow-ups proceeds as follows: the Z leads to one more identification such that, in the end, five deformations remain independent.
where Z 6 corresponds to the sector twisted by v + w.
Any factorisable bulk three-cycle takes the form [13], Π bulk a = P a 1 + Q a 2 + U a 3 + V a 4 with i = 2˜ i ⊗ π 5 , i+2 = 2˜ i ⊗ π 6 (P a , Q a , U a , V a ) = (X a n a 3 , Y a n a 3 , X a m a 3 , Y a m a 3 ) , 2 twisted sector has an identical basis upon permutation of two-torus indices. The number of independent complex structure deformations is thus reduced from 3 bulk + (3 × 16) Z 2 for T 6 /Z 2 × Z 2 with discrete torsion to 1 bulk + (6 + 2 × 4) Z 2 on T 6 /Z 6 × Z 2 with discrete torsion due to the Z 3 subsymmetry.
The multiplicities (h − 11 , h + 11 ) of Kähler moduli and closed string vector multiplets computed in [13] (cf. also table 2) provide a first hint that the choice of aor b-type lattice on T 2 (3) leads to physically inequivalent string models. The assumption of only two equivalent lattice backgrounds is further confirmed by a closer inspection of RR tadpole cancellation and supersymmetry conditions as well as massless open string spectra [60]. Focussing on the AAa/b formulation, the orientifold projection on the exceptional three-cycles at Z 2 fixed points is given in table 11, from which we can read off the h twisted 21 R-even cycles in dependence of the choice of exotic O6-plane. These are exactly the cycles to which the independent complex structure deformations in table 2 are associated.

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ΩR on exceptional three-cycles on T 6 /Z 6 × Z 2 on AAA 1, 2, 3 4, 5 Table 12. Orientifold projection of the exceptional three-cycles from the Z (k),k∈{1,2,3} 2 twisted sector on the AAA background of T 6 /(Z 6 × Z 2 × ΩR) with discrete torsion. In the example below η ΩR = −1 = η (k),k∈{1,2,3} is chosen.   Table 13. D6-brane data for a global Pati-Salam model on five stacks for η ΩR = −1 of the T 6 /Z 6 × Z 2 orientifold with discrete torsion. The corresponding gauge couplings g −2 SU(N )x ∝ Vol(Π a + Π a ) only depend on a subset of deformation moduli as displayed in the last column. ΩR-invariant orbit, but due to the choice τ e 1 = τ e 2 = 0 of discrete Wilson lines, the rigid three-cycle is not orientifold invariant. The associated gauge coupling only depends on the deformation moduli in the Z Open Access. This article is distributed under the terms of the Creative Commons Attribution License (CC-BY 4.0), which permits any use, distribution and reproduction in any medium, provided the original author(s) and source are credited.