Wilson-line Scalar as a Nambu-Goldstone Boson in Flux Compactifications and Higher-loop Corrections

We study a scalar zero mode originated from extradimensional components of a gauge field in a six-dimensional theory compactified on a magnetized torus. We confirm it is a Nambu-Goldstone boson of the translational symmetry on the torus which is breaking spontaneously due to magnetic flux. We also show explicitly it is massless up to the two-loop level. Moreover, we discuss full order contributions by considering the effective potential. ∗E-mail address : yakkuru 111@ruri.waseda.jp †E-mail address : tshd-sbsk.2015@ruri.waseda.jp ar X iv :1 91 2. 04 58 1v 1 [ he pth ] 1 0 D ec 2 01 9


Introduction
The Standard Model (SM) is the most successful model in particle physics. However, there are still many mysteries in the SM. For example, the origin of the chiral structure and the generation structure of fermions has not been revealed. These suggest the existence of physics beyond the SM.
Extradimensional models are one of the most interesting possibilities beyond the SM.
In particular, flux compactifications provide a lot of attractive results. In fact, fourdimensional (4D) chiral fermions and their generation structure can be realized by introducing magnetic fluxes in extradimensions [1]. Moreover, Yukawa couplings were computed explicitly in the magnetized models compactified on tori or toroidal orbifolds [2][3][4][5].
In extradimensional models, extradimensional components of gauge fields, which are often called Wilson-line (WL) scalars, are important since they can be candidates of 4D Higgs fields [6][7][8][9]. Recently, quantum corrections to the masses of WL scalars were calculated in flux compactifications. According to ref. [10][11][12][13], the quantum corrections vanish at the one-loop level with and without supersymmetry. This result is confirmed in a six-dimensional (6D) U(1) gauge theory [12] and an SU(2) gauge theory [13] compactified 1 on a torus T 2 with magnetic flux. In the previous researches, the physical reason for the cancellation of the mass corrections has been under discussion: the shift symmetry of the WL scalars [12] or Nambu-Goldstone (NG) bosons of the translational symmetry on a torus [10,13].
In this paper, we confirm in more detail that the WL scalar is an NG boson of the translational symmetry by considering commutation relations between the WL scalar and the momentum operators. We focus on a 6D U(1) gauge theory with a single Weyl fermion compactified on a magnetized torus as the simplest case. We calculate quantum corrections to the mass of the WL scalar and show the cancellation up to the two-loop level. To confirm its masslessness in the full order, we mention the effective potential does not depend on the value of the WL phase in our setup. This paper is organized as follows. In section 2, we explain the U(1) gauge theory on a magnetized torus. In section 3, we show the WL scalar is an NG Boson of the translations. In section 4, we calculate quantum corrections to the mass of the WL scalar. We summarize in section 5.
We take the metric as g M N = diag(−1, +1, · · · , +1), and define complex coodinates We introduce a left-handed 6D Weyl fermion Ψ interacting with a U(1) gauge field A M . The Lagrangian is given by where The third term is a gauge fixing term and ξ ≥ 0 is a gauge fixing parameter. 1 We summarize 6D gamma 1 This is an extension of the R ξ gauge in the SM.
2 matrices in appendix A. It is convenient to define a complex field φ as A constant magnetic flux f is given by the nontrivial background or VEVs of extradimensional components of the gauge field. In this paper, we introduce it as follows.
where θ 5,6 are constant WL phases. This configuration satisfies the classical equation of Accordingly, the VEV of the complex field φ is given as where θ = (θ 5 + iθ 6 ) /2. The magnetic flux is quantized on the torus, Using two-component Weyl fermions ψ and χ defined in appendix A, we can rewrite the Lagrangian (2) as follows.
where ϕ is a quantum fluctuation of φ around the VEV, In the following of this paper, we consider N > 0 without loss of generality. We define following operators, These satisfy the commutaion relations of creation and annihilation operators, [a, a † ] = 1, others = 0.
Mode functions of the two-component fermions are defined by these operators as where j = 0, · · · , |N | − 1 labels the degeneracy. 2 The WL phase θ shifts the position of the mode functions on the torus. These functions satisfy a orthonormality condition By use of this set of functions, the 6D fermions are Kaluza-Klein (KK) expanded, It is useful to define 4D left-handed Weyl fermions Ψ 0j and Dirac fermions Ψ nj , The KK expansions for bosons are given by where M lm = 2π (m + il). A µ,−l−m = A † µ,lm is satisfied since the gauge field A µ is real. The scalar zero mode ϕ 0 is called a WL scalar because the WL phase multiplied by an appropriate factor f θ/ √ 2 can be interpreted as its VEV. Before the dimensional reduction, we define 4D complex scalar fields η lm and σ lm when l or m is non-zero for convenience, 2 Explicit forms of the mode functions including massive modes are studied in ref. [14].

Substituting the KK expansions (15), (16), (18) and (19) into the Lagrangian (8) and
integrating it on a torus, we obtain the following 4D effective Lagrangian, where P L,R are 4D chirality projection operators and the coefficients are given by A lm nj,n j = with the overlap integrals When n or n is a negative integer, we define C lm nj,n j = 0. Here, C lm nj,n j is defined for the WL phase θ = 0 and independent of θ. In the 4D effective Lagrangian (22) and the following, the sum of l and m is in the following range, effective theory, respectively. The KK masses of NG bosons σ lm depend on the gauge fixing parameter ξ and they are eaten by the massive modes of the 4D vector fields A µ,lm as their longitudinal components.
By the definition of the overlap integrals, C lm nj,n j = C −l−m n j ,nj holds. The following recurrence relations are obtaind from the definition of the mode functions of the fermions, These equations are useful to calculate two-loop corrections in section 4.

Wilson-line Scalar as an NG Boson
The Lagrangian (8) Especially, this shift symmetry of the 6D field ϕ is rewritten to that of the WL scalar ϕ 0 in the 4D effective theory [12]. Therefore, the WL scalar in this setup is expected to be an NG boson of the translational symmetry.
To confirm this in more detail, let us consider commutation relations between the fluctuation ϕ and the Noether charges P z,z of the translations on the torus. Deriving the energy momentum tensor from the Lagrangian before introducing the magnetic flux, we obtain following terms containing ϕ, between P z,z and ϕ are given as follows.
The VEVs of them are This result implies the fluctuation ϕ is an NG boson of the translations. 3 Then, we show the WL scalar ϕ 0 takes over the property of the 6D field ϕ as an NG boson after the dimensional reduction. Substituting the KK expansion of ϕ into eqs. (32) and (33) and integrating them on the torus, we obtain the momentum density in the 4D effective theory, Commutation relations between P z,z and ϕ 0 are Therefore, In the 4D effectve theory, the WL scalar ϕ 0 is an NG boson of the translational symmetry on the torus.

Quantum Corrections
In section 3, we showed the WL scalar ϕ 0 is an NG boson. Therefore, it is expected to be massless in full order of the perturbation. In this section, we show it is true up to the two-loop level by diagrammatic calculations and in the full order from the WL phase independence of the effective potential. Feynman rules we use in the following are obtained from the 4D effective Lagrangian (22). First, we review the one-loop calculation [10,12]. Fig. 1 shows one-loop contributions to the mass of ϕ 0 . The sum of the loops over the mode of fermions is

One-loop Corrections
where an appropriate change of the integral variable is performed to simplify the masses in propagators. In the second to third line, we regularize the sum by the shift n → n + 1 in the second term. 4 We also use this reguralization method in the two-loop calculations.
Therefore, the WL scalar ϕ 0 is massless at the one-loop level.  . 2). The sum of these two-loops over the mode of fermions is
(44) Figure 4: Two-loop contributions including η lm as an internal line. Fig. 4 shows two-loop contributions including massive physical scalars η lm . We have to note there are three more types of diagrams where the direction of the scalar internal 10 line is flipped in addition to above three; that is, we consider six types of diagrams in total. The sum over the mode of fermions is where γ nn = n C lm nj,n −1j δ nn = n C lm nj,n −1j In this calculation, we use properties of the overlap integral C lm nj,n j such as eqs. (29) and (30). Note that we define C lm nj,n j = 0 when n or n is a negative integer. It is also shown that the sum of two-loop contributions including the NG scalars σ lm as an internal line is zero in the almost same way as above. there are also two choises of the direction of vector internal lines since A µ,lm is complex.
When the gauge fixing parameter ξ = 1, the sum of them is

Effective Potential
The WL phase with an appropriate factor f θ/ √ 2 is a VEV of the WL scalar ϕ 0 . Thus, its mass squared m 2 ϕ 0 is obtained as the second derivative of the effective potential V eff in the 4D effective theory respect to the VEV, In our setup, propagators or mass spectra in the 4D effective theory are independent of the WL phase θ. Furthermore, bubble graphs which contribute to V eff always include conjugate pare vertices proportional to e θM lm −θM lm or e −θM lm +θM lm . Thus, θ-dependence of vertices is cancelled in each bubble graph and V eff is independent of θ. Therefore, the WL scalar is massless in the full order.
Because of θ-independence of V eff , a mechanism which dynamically determines the value of the WL phase, i.e. the Hosontani mechanism [8,9], does not work in our setup.

Summary
In this paper, we have studied properties of the WL scalar in a 6D U(1) gauge theory compactified on a torus with magnetic flux. In the previous researches, it has been shown that the quantum corrections to the masses of the WL scalars vanish at the one-loop level in a few gauge theories on a magnetized torus. The physical reason for this masslessness has been discussed to be the shift symmetry of the WL scalars or that they are NG bosons of the translations on the torus.
First, we derived the 4D effective Lagrangian including the WL phase from the dimensional reduction of U(1) gauge theory on M 4 × T 2 with magnetic flux. The main target of this paper was a scalar zero mode originated from the extradimensional components of the gauge field.
The translational symmetry on the torus is breaking spontaneously due to magnetic flux. To confirm the WL scalar is an NG boson of this translations, we computed commutation relations between the WL scalar and the momentum operators. In the 6D theory, extradimensional components of the gauge field are NG bosons and their property as NG bosons is taken over by the WL scalar after dimensional reduction.

13
Using the 4D effective Lagrangian, we have calculated quantum corrections to the mass of the WL scalar up to the two-loop level. The corrections cancel non-trivially by summing up contributions from all the fermion KK modes. To confirm the masslessness of the WL scalar, we have also discussed the effective potential. Since it is independent of the WL phase, the WL scalar is indeed massless in the full order. In addition, the WL phase is not determined dynamically like some gauge-Higgs unification (GHU) models.
In this paper, we have focused only on a 6D U(1) gauge theory compactified on a magnetized torus. It would be interesting to confirm the cancellation of higher-loop corrections in other gauge theories or to generalize this result to flux compactifications on other manifolds.
Since massless scalars are phenomenologically undesirable, we are also interested in how to make the WL scalars massive, that is, pseudo-NG bosons without spoiling desirable results of flux compactifications such as the chiral structure and the generation structure of fermions. If it is possible, the application to GHU models might be interesting.

Acknowledgments
We would like to thank Hiroyuki Abe for useful comments and discussions.

A. Gamma Matrices
The gamma matrices we used in this paper satisfy the 6D Clifford algebra Our choice for 6D gamma matrices are where the 4D gamma matrices are given by In this notation, the 6D chirality operator is given by 14 For these gamma matrices, we can decompose a left-handed 6D Weyl fermion Ψ into two-component Weyl fermions ψ and χ as follows.