Quantum Wilson surfaces and topological interactions

We introduce the description of a Wilson surface as a 2-dimensional topological quantum field theory with a 1-dimensional Hilbert space. On a closed surface, the Wilson surface theory defines a topological invariant of the principal G-bundle P → Σ. Interestingly, it can interact topologically with 2-dimensional Yang-Mills and BF theories modifying their partition functions. This gives a new interpretation of the results obtained in [1]. We compute explicitly the partition function of the 2-dimensional Yang-Mills theory interacting with a Wilson surface for the cases G = SU(N)/ℤm, G = Spin(4l)/(ℤ2 ⊕ ℤ2) and obtain a general formula for any compact connected Lie group.


Introduction
The discussion of surface observables in gauge theories has been ongoing for quite some time. Wilson surfaces, domain walls, surface defects etc appear in many domains of physics and mathematics, from gauge theories to condensed matter. They have been studied extensively in literature [2][3][4][5][6][7][8]. In most cases a 1-dimensional observable, namely a Wilson line [9][10][11][12][13][14][15][16][17], is generalized to 2 dimensions by introducing higher gauge fields defined on surfaces. Our approah is different, it is based as well on a definition of a Wilson line, but doesn't involve introducing higher gauge fields.
The first result of this article is a formulation of the Wilson surface as a new 2dimensional topological quantum field theory. We define its action, the Hilbert space and compute its partition function.
The basis for our construction is a 1-form standard gauge field taking values in a Lie algebra. A Wilson surface is defined by an orientable surface Σ and an irreducible representation R λ of the gauge group G. In [1] we obtained its description as a 2-dimensional topological σ-model: where λ ∈ Λ * is the highest weight of the representation R λ , b is a scalar field taking values in g * and constrained to be a conjugate of λ ∈ Λ * , A is a background gauge field, and a is an auxiliary gauge field. Interpreting A + a as a new gauge field allows us to JHEP02(2019)030 interpret a Wilson surface as an independent 2-dimensional BF-theory with a constraint on the B-field.
In this article we start with the action functional (1.1) from [1] and canonically quantize it to obtain the partition function formula for the Wilson surface theory. To describe the formula we first recall some topological facts. Principal G-bundles P → Σ over a closed surface Σ are classified by the elements γ ∈ π 1 (G) in the fundamental group of the gauge group G [18,19]. The gauge group can be represented as G =G/Γ, whereG is the universal cover of G and Γ ⊂ Z(G) is a proper subgroup of the center ofG. Since Γ ∼ = π 1 (G), for every element γ ∈ π 1 (G) in the fundamental group there exists a corresponding element C γ ∈ Γ ⊂ Z(G) in the center of the covering group. Then the partition function for a particular equivalence class of principal bundles P → Σ, defined by γ ∈ π 1 (G), is given by: where χ λ (C γ ) is a value of the character χ λ on the element C γ and d λ is the dimension of the representation. This is a 2-dimentional topological quantum field theory with a 1-dimensional Hilbert space.
Our second result is the description of topological interactions of Wilson surfaces with 2-dimensional topological gauge theories, e.g. with BF or Yang-Mills theories. Their partition functions on a surface Σ are obtained by summation over all the classes of principal G-bundles defined over the given surface [20][21][22]. When we insert a Wilson surface into 2dimensional BF or Yang-Mills theory, it interacts topologically with the background gauge theory, as the gauge connections A and A + a are defined on the same principal G-bundle P → Σ. The presence of a Wilson surface modifies the partition function of the background theory multiplying by a phase (1.2) the individual contributions for each class of principal bundles: (1.3) In subsection 3.1 we describe explicitly the action and the partition function of 2dimensional BF-theory interacting with the Wilson surface theory.
The formulas of the partition function for 2-dimentional Yang-Mills theory with an insertion of the Wilson surface observable were first obtained in [1] for the cases of G = U(1), SU(2), SO(3). In subsection 3.2 of the current article we write the general formula for 2-dimensional Yang-Mills theory with a Wilson surface and give it a new interpretation of the topological interaction.
Since Yang-Mills theory in 2 dimensions is exactly solvable, we can compute explicitly the partition functions in the presence of a Wilson surface for concrete gauge groups. The examples of G = U(1), SU(2), SO(3) were computed in [1]. In this article we compute the partition functions of 2-dimensional Yang-Mills theory with a Wilson surface for a larger class of gauge groups. In particular, we study in detail the examples of the gauge groups G = SU(N )/Z m (m divides N ) and G = Spin(4N )/(Z 2 ⊕ Z 2 ).

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In case of G = SU(N )/Z m the fundamental group is π 1 (G) ∼ = Z m and the Wilson surface phase e iϕ k is defined by the angle: where k = 0, 1, . . . , m − 1 labels the elements of π 1 (G), and [λ] ∈ Z m is an integer mod m denoting the equivalence class of the highest weight λ characterising the Wilson surface. For G = Spin(4N )/(Z 2 ⊕ Z 2 ) the fundamental group is π 1 (G) ∼ = Z 2 ⊕ Z 2 and the Wilson surface is defined by the angle: where a pair (k 1 , k 2 ) labels the elements of π 1 (G), with k 1 , k 2 ∈ {0, 1}, and [λ 1 ], [λ 2 ] ∈ Z 2 are integers modulo 2 given by two linear combinations of the components of same highest weight λ characterizing the Wilson surface. Eventually, we obtain the formula of the partition function for 2D-YM with a Wilson surface for any compact connected Lie group G =G/Γ. In this case the Wilson surface phase is defined by the angle: Here we account for the most general case, when the fundamental group of G is given by a product of i cyclic groups: is an element of the Cartan subalgebra such that e i i k i c i = C k 1 ,...,k i ∈ Γ ∼ = π 1 (G) is a central element of the covering groupG, λ ∈ h * is the highest weight of the irreducible representation of G characterizing the Wilson surface, <, > is the invariant scalar product defined on Lie(G) and [λ i ] ∈ Z m i are integers modulo m i given by i linear combinations of the components of same highest weight λ. For a closed surface the Wilson surface is nontrivial for G non-simply connected, and it is not visible (e iϕ = 1) for G simply connected. Also the value of λ plays a role: for λ being the highest weight of a representation of the gauge group G itself the Wilson surface is trivial, and it is nontrivial if λ labels a representation of the universal coverG which does not descend to G. On a closed surface, the partition function of the Wilson surface is a topological invariant of the principal G-bundle.

Wilson surface observables
Recall the construction of Wilson surface observables from [1]. Let G be the gauge group, g its Lie algebra, (x, y) → Tr(xy) an invariant scalar product on g and P a principal Gbundle over a surface Σ. We denote by h ⊂ g a Cartan subalgebra and by Λ * ⊂ h * the weight lattice.
A Wilson surface observable is described by an auxiliary 2-dimensional gauge theory on the surface Σ. The fields in this theory are a g * -valued scalar field b and a g-valued 1-form a. The action depends on the following data: the background gauge field A and the weight λ ∈ Λ * . For a trivial G-bundle it is given by where we identified g * with g using the scalar product and integrated by parts using the equality Trb[dgg −1 , a] = Tr[b, dgg −1 ]a = −Tr(db)a. The field b = gλg −1 belongs to the same conjugacy class as the fixed element λ, the combination A + a is a new gauge field. The fields obey the following gauge transformation rules: by h : Σ → G they transform as Note that integrating out a in (2.1) yields the Diakonov-Petrov action [1,23] for a Wilson surface: The construction (2.1) also works on nontrivial bundles. A ∈ Ω 1 (P, g) is the connection on P , its curvature F A ∈ Ω 2 hor (P, g) G is a horizontal 2-form taking values in g. The auxiliary gauge field a is such that a ∈ Ω 1 hor (P, g) G and the sum A + a defines a new connection on P with a curvature F A+a = d(A + a) + (A + a) 2 , F A+a ∈ Ω 2 hor (P, g) G . The field b takes values in Ω 0 hor (P, g * ) G . The combination Tr(bF A+a ) is then a basic 2-form which decends to Σ. One can show this in the following way. The 2-form bF A+a is G-equivariant, i.e. under the gauge transformations it transforms as b h F A h +a h = hbF A+a h −1 , yeilding Tr(b h F A h +a h ) = Tr(bF A+a ). Acting by the contraction we obtain: where ξ ∈ g induces the fundamental vector field ξ ∈ X(Σ), and we have used that ı ξ (dg) = −ξg, ı ξ A = ξ (by definition of connection), ı ξ F A = 0, ı ξ a = 0 (F A and a are horizontal). This computation proves that G-invariant form Tr(bF A+a ) is horizontal, and hence basic.
The meaning of λ ∈ Λ * + is as follows. The integral weights of the representations of G form the weight lattice Λ * ⊂ h * . Dominant integral weights Λ * + ⊂ Λ * are in one to one

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correspondence with irreducible representations of G [24,25]. The element λ ∈ Λ * + is the highest weight of some representation of G, it is a parameter characterising the Wilson surface. For example, for G = SU(2) or G = SO(3) we talk about a Wilson surface of spin λ. Note that in case when G is not simply connected but is a quotient G =G/Γ, whereG is its universal cover and Γ ⊂ Z(G) is a subgroup of the center ofG, the weight lattices are related as Λ * G ⊂ Λ * G . A representation ofG can be considered as a projective representation of G, and λ is allowed to take values in Λ * G , and, as we will see later, these are exactly the values which describe the presence of nontrivial Wilson surfaces.

Quantum Wilson surfaces
The action for a Wilson surface (2.1) was first constructed in [1] to represent a surface observable within some other gauge theory. In the current paper we define it to be a separate 2-dimensional quantum field theory. Its action is a 2-dimensional BF theory [26] on Σ, with respect to the new connection A + a: There is just one subtlety which distinguishes the Wilson surface theory from an ordinary BF-theory: its b-field, as described in the previous subsection, is restricted to take values in the coadjoint orbit of λ, O λ ⊂ g * . This affects, as we will see later, the definition of the Hilbert space of the Wilson surface and the structure of its partition function. Nevertheless, as a starting point for our formulation we recall canonical quantization of an ordinary BFtheory on a surface and the derivation of its partition function first done by Migdal in [27] and then discussed in more detail by Witten in [20,21]. 1 For simplicity let first Σ be a cylinder C, the G-bundle P will be necessarily trivial. We chose space and time coordinates (x, t) in a way that the boundary of C is given by two closed curves γ 1 and γ 2 , situated on equal time slices, and x is a periodic coordinate of period L. We associate to γ i a gauge invariant wave function ψ(A) which is a function of holonomy U i of A around γ i : The Hilbert space H γ of such a theory is given by G-invariant L 2 functions on G. H γ admits a natural basis in terms of characters of representations, and any wave function ψ(A) ∈ H γ has an expansion in characters χ R (U ), where R is an irreducible representation. The boundaries are oriented, the wave functions on the incoming and outgoing boundary components are denoted by χ R (U i ) and χ R (U j ) respectively.
In BF-theory the Hamiltonian vanishes (as expected for a topological field theory), so the partition function on a cylinder (equation 4.12 in [21]) reduces to:

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For a generic surface with genus g and r boundary components the BF partition function (equation 2.68 in [20]) reads: where d R is the dimension of the irreducible representation R and all the boundaries are chosen to be outgoing. To obtain the formula for a closed surface we proceed as follows. The partition function will necessarily depend on the equivalence class of G-bundle over Σ. Recall the classification of principal G-bundles over Σ by the elements of the fundamental group of G: π 1 (G) ∼ = Γ ⊂ Z(G). Consider a surface with just one puncture, i.e. one boundary component. Gluing this puncture to an infinitesimal disc yeilds a closed surface, and this operation is described The contribution to the partition function of each class [P ] of a principal G-bundle over the surface is given by (equation 4.26 in [21]): The total partition function for BF-theory on a closed surface Σ is then a sum over equivalence classes of principal G-bundles over Σ (equation 4.27 in [21]): where #Γ is the cardinality of Γ. Note that the sum over R in (2.7) converges only for surfaces Σ with genus g > 1.
Using the tools from [20,21] described above we can now define our Wilson surface theory. It is a very simple 2-dimensional gauge theory and in what follows we are going to explain how to construct its partition function. In contrast with BF-theory, the g *valued field b = gλg −1 is now the conjugation of the same fixed element λ ∈ Λ * G . The Hilbert space becomes one-dimensional choosing just one irreducible representation R λ , and the partition function is just a phase. The normalization of the states is such that Any orientable surface can be obtained by gluing together some elementary components, namely discs and pairs of pants. So it is sufficient to define the states corresponding to these elementary components and then the definition of the Wilson surface for any orientable surface will follow. A natural way to describe the state corresponding to a disc would be to assign a character of holonomy U of the connection A + a to the boundary of the disc and a character of the identity element e of the holonomy group to the second "no-boundary" of the disc. This formulation was chosen by Witten in [20,21], and it would give the following: where the orientation is chosen in a way that U is a holonomy of the connection A+a around an outgoing boundary, and e is a holonomy around an incoming boundary. In contrast with

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BF-theory this formulation is not good for our Wilson surface with a 1-dimensional Hilbert space for the following reason: the value of the character of the identity χ λ (e) yields the dimension of the representation, so the state Z disc o (U, λ) will not satisfy the normalization condition || < χ λ (U )|χ λ (U ) > || 2 = 1. This motivates us to introduce a normalization factor 1 d λ into the definition of the disc state: where d λ is the dimension of the irreducible representation corresponding to the highest weight λ. The Wilson surface on a pair of pants is naturally defined by the formula: where U 1 , U 2 , U 3 are holonomies of A + a around one incoming and 2 outgoing boundary components.
Then any other orientable surface can be obtained by gluing those components together, i.e. assigning the same holonomy element U i to the incoming and outgoing boundaries which we want to glue, and integrating over it using the property of the characters: The partition function for a surface of arbitrary genus with r boundary components is thus a product of r states living on the boundaries (here chosen to be outgoing): To get the expression for a closed surface we start with a surface with one boundary component Z Σ W S (U 1 , λ) = χ λ (U 1 ) and glue it to a disc Z disc W S (U 1 , λ) = χ λ (U 1 ) χ λ (e) d λ , the factor χ λ (U 1 ) disappears after the integration. But here there is a subtlety: unlike over an open surface, a principal G-bundle over a closed surface in general can be nontrivial, so, keeping the normalization factor 1 d λ , we replace the identity element of holonomy e by a central element C i corresponding to a particular class [P ] of the bundle P → Σ. This yields the formula of the Wilson surface theory for a closed surface for a class [P ] of principal bundles P → Σ: For a nontrivial central element C i this is an element of U(1): Z Σ W S (C i , λ) ∈ U(1). In case when P is a trivial bundle, the Wilson surface is always trivial: Z Σ W S (P triv , λ) = 1.

Topological interactions with 2-dimensional gauges theories
In general case our observable could be understood as a surface defect embedded into a higher dimensional space-time. But in this paper we want to test it in the context of 2dimensional gauge theories, which can be solved exactly. In this case the Wilson surface is a "global" observable, defined on the entire 2-dimensional space-time Σ.

BF-theory with a Wilson surface
The action functional for BF-theory with a Wilson surface is: where B ∈ Ω 0 (P, g * ) G , A ∈ Ω 1 (P, g) is the background gauge field, F A ∈ Ω 2 hor (P, g) G its curvature.
These two BF-theories are not completely independent, they interact topologically: the connections A and A + a are defined on the same principal G-bundle, so the characters χ R (U(A)) and χ λ (U(A + a)) are taken on the same central element.
Then the partition function for a closed surface with a Wilson surface of weight λ is obtained by taking a product of partition functions (2.6), (2.11) defined in the previous section for each class [P ] and then summing over all the equivalence classes:

2D-YM theory with a Wilson surface
In this subsection we derive of the partition function for 2D-YM with a Wilson surface observable. In [1] the partition function formulas were obtained for the cases of U(1), SU(2) and SO (3) where B is an auxiliary field taking values in g * and d 2 σ is the area element on Σ. Again, we see that the action splits into two theories interacting topologically through the connections A and A + a defined on the same principal bundle. The partition function for each class [P ] will be a product of the partition function for 2D-YM and the partition function for the Wilson surface. Canonical quantization of this interacting theory goes as follows. The Hamiltonian of the first theory is H = e 2 2 TrB 2 . The Hamiltonian of the second theory vanishes. The basis for the Hilbert space, as it was described in [1], is given by gauge invariant functions

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Then the time evolution operator takes value e −τ C 2 (R) on the functions ψ R (A, a), where τ = e 2 2 σ absorbs the YM coupling constant e 2 and the area of the surface σ.

First, we obtain the partition function for each class [P ] which is a product of a Wilson surface phase (2.11) and the 2D-YM partition function
Then the total formula of the partition function for a closed surface with a Wilson surface of weight λ is given by the sum over all the equivalence classes [P ]:

Exact results for 2D-YM theory interacting with a Wilson surface
Yang-Mills theory in 2 dimensions is exactly solvable [27][28][29][30][31][32][33][34][35][36], this allows us to obtain explicit formulas for the partition function in the presence of a Wilson surface. In [1] we computed the partition functions for 2D Yang-Mills with a Wilson surface for the gauge groups U(1), SU(2) and SO (3). Now we are going to generalize this result to G being any compact connected Lie group.

SU(N) and the groups covered by SU(N)
To n=1 a n h n , with a n ∈ R linear coefficients. Exponentiating elements h ∈ h we obtain the maximal torus of SU(N ): H = e ih = e i anhn = diag(e iθ 1 , e iθ 2 , . . . , e iθ N−1 , e −i N−1 i=1 θ i ) ∈ T. The center Z(SU(N )), and hence its proper subgroup Γ ⊂ Z(SU(N )) ⊂ T , is a subgroup of the maximal torus: Γ C k = e iθ k Id N ∈ T , with θ k = 2πk/m.
Consider the elements of the Cartan subalgebra c k = diag(θ k , θ k , . . . , −(N−1)θ k ) N×N ∈ h, such that C k = e ic k ∈ Z(SU(N )). In terms of the basis of h they are given as follows: Then the central elements of SU(N ) are given by C k = e iθ k N −1 n=1 nhn ∈ Z(SU(N )). The irreducible representations of SU(N ) are labeled by highest weights with N − 1 independent elements: µ = (µ 1 , . . . , µ N −1 ).
The central elements in the representation R µ of highest weight µ are obtained as: R µ (e iθ k N −1 n=1 nhn ) = e iθ k N −1 n=1 nRµ(hn) . The natural choice for the basis of R µ is in terms of the weight vectors. In this basis R µ (h n ) are diagonal and yield weights while acting on the basis vectors. A central element

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C k is a multiple of identity, therefore R µ (C k ) has to be a multiple of identity as well, so it's enough to compute it just on the highest weight vector: (4.1) The linear combination N −1 n=1 nµ n is an integer, but the expression (4.1) depends only on the value of this sum modulo m, as e i 2πk . This allows us to define the equivalence classes of the highest weight µ: Note that the irreps ofG descend to the irreps of G if N −1 n=1 nµ n = 0 mod m. In terms of weight lattices Λ * G ⊂ Λ * G ⊂ h * , where Λ * G is the weight lattice for SU(N ), Λ * G is the weight lattice for G = SU(N )/Z m .
The characters of the central elements in the representations R µ are as follows: We keep the notation Z Y M (τ ) for the partition function of the free 2D-YM theory and Z λ Y M (τ ) for the theory with a Wilson surface of the highest weight λ. Without Wilson surface the partition function for SU(N )/Z m is given by where the sum is over the representations R µ of SU(N ), and k labels central elements in the subgroup Γ. The computation gives the following result: where the sum over k is equal to m for [µ] = 0 and zero otherwise. The condition corresponds to those representations of SU(N ) in which the central elements are all trivial, that is to the representations of SU(N )/Z m :
The sum over k in (4.7) is different from zero only for [µ] + [λ] = 0, and the partition function formula for 2D-YM with a Wilson surface yields: where the sum now goes over the representations R µ+λ of G = SU(N )/Z m of highest weights µ + λ, i.e.
[µ] = [−λ] ∈ Λ * G /Λ * G . Note that in case when G = SU(N ), i.e. the gauge group is simply connected, the presence of the Wilson surface makes no impact on the partition function. Let us look at this situation in more detail. There is just one class of principal SU(N )-bundles over a surface Σ -trivial SU(N )-bundle. The SU(N ) partition function without Wilson surface is given by: where e is the identity. And adding a Wilson surface of weight λ leaves the partition function unchanged:

Generalization for any compact connected Lie group
The result explained in the explicit example of the previous section remains valid for all compact connected Lie groups. All of them (with the exception of exceptional ones) have as a universal cover one of the following groups: SU(N ), Spin(N ), Sp(N ) and can be obtained by taking a quotient by a subgroup Γ of the center.

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The case ofG = SU(N ) has been discussed in the previous section. For Spin(N ), N ≥ 3 the data is as follows: (4.10) The group Sp(N ) has the center Z(Sp(N )) = Z 2 . Among the exceptional groups only E 6 and E 7 are interesting for our purposes, the rest of them (G 2 , F 4 and E 8 ) are simply connected and have a trivial center. The real compact forms of E 6 and E 7 are not simply connected. The universal cover of E 6 has the center Z(Ẽ 6 ) = Z 3 , and the universal cover of E 7 has the center Z(Ẽ 7 ) = Z 2 .
We consider the gauge group G =G/Γ. The center of the cover Z(G) ⊂ T is a subgroup of the maximal torus. T is given by the elements H = e ih ∈ T , where h ∈ h is in the Cartan subalgebra.
The irreducible representations ofG are labeled by highest weight with n independent elements, where n is the rank ofG: (µ 1 , . . . , µ n ).
In most cases the center ofG, or its proper subgroup Γ, is given by Z m for some m ∈ Z, and the calculation looks similar to theG = SU(N ) example. But in general Γ can be represented by a product of i cyclic groups: Γ = Z m 1 × . . . . × Z m i . We take the elements i k i c i ∈ h in the Cartan subalgebra h ofG and exponentiate them to get the central elements C k 1 ...k i = e i i k i c i ∈ Z(G). Here we account for the structure of Γ: the index i refers to the i-th factor in the product and the coefficient k i labels the elements inside each factor Z m i .
In terms of the basis of the Cartan subalgebra h j ∈ h we can express The representation R µ of a central element C k 1 ,...,k i is given by the formula: The characters of the central elements in the representations R µ are: (4.11) Here we have rewritten the pairing i k i < µ, c i > in the following way: where (a i ) j are linear coefficients producing different linear combinations of µ j s for each k i -th element. The i different linear combinations n j=1 (a i ) j µ j ∈ Z define i types of equivalence classes of the highest weight µ: is an integer modulo m i . Without Wilson surface the partition function for G is given by: Rµ e −τ C 2 (Rµ) χ Rµ (C k 1 ,...,k i ), (4.12)

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where the sum is over the representation R µ of G =G/Γ and i coefficients k i label a central element in the subgroup Γ.
Using (4.11) we compute: (4.14) Now let us introduce a Wilson surface of weight λ. Just like any highest weight, λ will belong to i types of equivalence classes defined by the pairing k i < λ, c i >= 2π k i m i n j=1 (a i ) j λ j , where (a i ) j are real linear coefficients for the pairing with the k i -th element and n j=1 (a i ) j λ j is an integer. Then the weight λ will be characterised by belonging to i types of equivalence classes: The partition function with a Wilson surface of weight λ is given by: where the sum is over such representations R µ (G), that the representations ofG with the highest weight µ + λ would correspond to the representations of G =G/Γ.

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Now let us illustrate the formulas (4.15), (4.16) with an example of a gauge group with π 1 (G) ∼ = Γ = Z m 1 × . . . × Z m i . The covering groupG = Spin(4l) has the center given by a product of two copies of Z 2 : Z(Spin(4l)) = Z 2 ⊕ Z 2 . If we factorize by the entire center we get G = Spin(4l)/Z 2 ⊕ Z 2 . We start with the central elements ofG = Spin(4l): in the Cartan subalgebra of Spin(4l), the coefficients k j = 0, 1 label the elements in the j-th copy of Z 2 , and (a 1 ) i , (a 2 ) i are real coefficients describing the elements c 1 and c 2 respectively and depending on the choice of a basis h i .
Without Wilson surface the partition function for G = Spin(4l)/Z 2 ⊕ Z 2 is given by:  In more detail, the sum in the first line of (4.18) runs over the representations R µ of Spin(4l) and in the last line -over the representations R µ of Spin(4l)/(Z 2 ⊕ Z 2 ). The change happens for the following reason. Each sum over k i in the second line is equal to zero, or to 2 if n i=1 a i µ i is even, i.e. [µ i ] = 0. This condition corresponds to chosing only those representations of Spin(4l) in which the elements C k 1 k 2 ∈ Z 2 ⊕ Z 2 are all trivial, i.e. the representations of Spin(4l)/(Z 2 ⊕ Z 2 ).
When we introduce a Wilson surface of weight λ, it will involve defining two equivalence classes for λ from the pairing < λ, k i c i >: Here the sum over each k i is different from zero only for µ i + λ i even. This condition reduces the sum in the last line to the sum over such representations R µ (Spin(4l)) that the representations of Spin(4l) with the highest weight µ + λ would correspond to the representations of Spin(4l)/(Z 2 ⊕ Z 2 ).
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