Tensor polarizability of the vector mesons from SU(3) lattice gauge theory

The magnetic dipole polarizabilities of the vector ρ0 and ρ± mesons in SU(3) pure gauge theory are calculated in the article. Based on this the authors explore the contribution of the dipole magnetic polarizabilities to the tensor polarization of the vector mesons in external abelian magnetic field. The tensor polarization leads to the dilepton asymmetry observed in non-central heavy ion collisions and can be also estimated in lattice gauge theory.


Introduction
The influence of strong magnetic fields on quark-hadron matter represents rich and full of surprising effects area of science. These fields could exist in the Early Universe, they can influence the physics of neutron stars, and lead to non-trivial effects in non-central heavy-ion collisions in terrestrial laboratories. Behaviour of the hadron energy in external magnetic field may provide information about the particle internal structure. In strong magnetic field the hadronic wave function deforms. This deformation is defined both by QED and QCD interactions inside the hadron. The magnetic polarizability and hyperpolarizabilities are quantities describing the response of the hadron to the external magnetic field, which we have explored in our previous work [1]. Apparently, this non-linear response arises solely due to the strong QCD interaction binding quarks together.
Below we discuss the calculations in lattice gauge theory with chiral invariant Dirac operator without dynamical quarks. Our method enables to calculate the hadronic energies for different spin projections on the magnetic field axis. Magnetic polarizabilities and moments can be extracted as the fit parameters from the magnetic field value dependence of the energy. The values of the magnetic polarizabilities depend on the meson spin projection on the field axis. The physical meaning of this phenomenon is related to different deformations of a hadron in the various space direction. Therefore, the presence of a magnetic field JHEP11(2018)186 creates a kind of anisotropy in space, which can lead to tensor polarization (alignment) of the vector meson and, after its decay, to dileptonic asymmetry in collisions of heavy ions. Dilepton anisotropy [24] is an important physical characteristic which is sensitive to different channels of particle's decay and can be utilized to disentangle contributions of some channels. Dilepton asymmetries provide information about the evolution of quark-gluon plasma in non-central heavy-ion collisions [25]. Here we study the influence of magnetic field on the tensor polarization of ρ mesons which was detected in angular distribution of their decay products. This requires a more accurate calculation of polarizability, so, we repeat we repeat, improve and extend our previous analysis [1,11].
The calculations were carried out in SU(3) lattice gauge theory without dynamical quarks. We consider the lattice volumes N t × N 3 s = 18 4 and 20 4 and a set of lattice spacings a = {0.095, 0.105, 0.115} fm. In table 1 we show the lattice volume N t × N 3 s , the lattice spacing a, the corresponding β imp values and the number of configurations.
In order to construct meson correlation function, we used quark propagators, which can be extracted as a series of eigenfunctions and eigenvalues of discrete lattice version of the Dirac operator.
where M = 50 is used for the calculations. The next step is the numerical solution of the Dirac equation and finding the eigenfunctions ψ k and the eigenvalues λ k of the Dirac operator for a quark located in an external JHEP11(2018)186 In these calculations we used the Neuberger overlap operator [28]. This operator enables to consider the limit of massless quarks without breaking the chiral symmetry and can be written in the following form where D W = M − ρ/a is the Wilson-Dirac operator with the negative mass parameter ρ/a, a is the lattice spacing, M is the Wilson term. The sign function sign(H W ) of the Hermitian Wilson-Dirac operator H W is determined by the following relation It is calculated using the min-max method of approximation by polynomials. The fermionic fields satisfy the periodic boundary conditions in space and the antiperiodic boundary conditions in time. We investigate the behaviour of the ground state energy of the meson in a gauge field, which is the sum of the gluonic field and the external constant magnetic field. The magnetic field interacts only with quarks, so the magnetic field was added only into the Dirac operator. A constant magnetic field B is directed along the z-axis The quantization of the magnetic field on a torus was originally discussed in [29][30][31]. In order to satisfy the boundary conditions for fermions, the magnetic field has to be quantized on the lattice [32] qB = 2πk (aN s ) 2 , k ∈ Z, (2.8) where q = −1/3 e, aN s is the lattice space extension. The calculation of the eigenfunctions and eigenvalues of the Dirac operator allows us to find the value of the two-point correlation function by means of which we determine the energy of the ground state.

Meson correlation functions
We calculate the following correlation functions where γ i , γ j are the Dirac gamma matrices with the Lorentz indexes i, j = 1, 2, 3 x = (na, n t a) and y = (n a, n t a) are the coordinates on the lattice. The spatial coordinates on the lattice are written as follows: n, n ∈ Λ 3 = {(n 1 , n 2 , n 3 )|n i = 0, 1, . . . , N − 1}, n t , n t are the numbers of sites in the time direction. In the Euclidean JHEP11(2018)186 space ψ † =ψ. The correlators of the ρ ± mesons (3.1) are computed with the use of the relation where D −1 d and D −1 u are the propagators of the d and u quarks in the coordinate space. We consider the isospin symmetry case, so at zero magnetic field D −1 d = D −1 u , but at non-zero field this equality is not fulfilled.
Since the u and d quarks interact differently with the field, the correlator of the ρ 0 meson is represented by the sum We numerically perform Fourier transform of the correlators from the coordinate space to the momentum space. In order to find the ground-state energy, we consider mesons with zero spatial momentum.
The ground-state energy of a meson with a definite spin projection on the magnetic field axis is defined by the covariant density matrix. We express the spin density matrix in terms of transverse (e x = (0, 1, 0, 0), e y = (0, 0, 1, 0)) and longitudinal (e z = (0, 0, 0, 1)) polarization vectors. Then the energies of the ρ ± and ρ 0 mesons with the spin projection s z = 0 are obtained from equations (3.2) and (3.3) respectively after Fourier transform, where i, j = 3.
The combinations of the correlators give the energies of vector mesons with the spin projections equal to +1 and −1 on the field axis, where are the interpolation operators of the ρ ± mesons. The interpolation operators for the ρ 0 case are constructed similarly to (3.4) taking into account (3.3).
The correlation function can be expanded in a series over the eigenstates of the where i, j = 1, 2, 3, E m and E n are the energies of the excited states with the numbers m and n, and Z = n n|e −T H |n = n e −T En is the partition function. In expression (3.5) we take out the factor e −T E 0 , as a result, we obtain the following relation

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where ∆E n = E n − E 0 . In the thermodynamical limit of the theory T → ∞ from (3.6) we obtain In our case we got the following expression One can see from (3.8) that at-large n t the main contribution comes from the ground state. Taking into account periodic boundary conditions on the lattice we obtain the final formula where A 0 is the constant, E 0 is the ground state energy. We use this formula for fitting the correlation functions obtained from the lattice propagators. From this fits the ground state energies can be obtained.

Calculation of m eff and its statistical errors
The ρ-meson effective masses m eff were extracted from χ 2 -fits to the standard asymptotic parametrization (3.9), with fit parameters being m eff = aE 0 and A 0 . The effective mass can be also found from the following equation: in which the boundary conditions on the lattice are taken into account. We have checked that the results for the energies coincide with the results obtained from (4.1), taking into account the correlation matrix between the adjacent points of the plateau. In order to control the stability of resulting m eff values, i.e. to determine the m eff (n t ) plateau, the fits were performed in four ranges of n t = N T 2 − k, N T 2 + k , k = 1 . . . 4, where the fit quality could be satisfactory, Despite that the fit quality was often acceptable already at k 4, the values of m eff at k = 4 could still be systematically overestimated.
Usually, the m eff plateau was reached at k = 3, i.e. n t = 6 ÷ 12 (7 ÷ 13) for lattice volume 18 4 (20 4 ). In some cases a narrower n t range was conservatively chosen after a visual inspection of the fits to ensure that m eff was well within the plateau. A typical graph of m eff (ρ 0 ) depending on the fit range n t is shown in figure 1 for the lattice volume 18 4 , the lattice spacing a = 0.115 fm, spin projections |s z | = 0, 1 on the magnetic field axis and two values of the magnetic field.
The uncertainties attributed to the resulting ρ-meson effective masses m eff are statistical-only, as determined by the fit in the chosen n t range.

Magnetic polarizabilities of the ρ ± mesons
In the magnetic field the energy levels of the point-like charged particle are described by the following dependency [33] where p z is the momentum in the magnetic field direction, n is the principal quantum number, q is the particle electric charge, g is the g-factor, s and m are the particle spin and mass respectively. As we discussed earlier [1] the magnetic field can affect the internal structure of vector mesons if it is sufficiently strong. This influence is characterized by non-zero magnetic polarizabilities and hyperpolarizabilities which depend on the projection of the meson spin s z on the direction of the magnetic field. It means that the response of the fermionic currents inside the meson is defined by the mutual orientation of the quarks and the external magnetic field. These phenomena are interesting and can give a contribution to the polarization of the emitted charged particles in the strong magnetic field which we discuss below.
According to the parity conservation for the spin projection s z = 0 the energy squared gets corrections from the non-linear terms of even powers in a magnetic field. For the spin projections s z = +1 and s z = −1 the energy squared contains the terms of both even and odd powers in the field. We found the contributions of these terms depend on the interval of magnetic fields considered. So, for the lattices considered the correction of the third power term to the lowest energy sub-level with qs z = +1 is not larger than 20% and compatible with errors at eB ∈ [0, 1.2] GeV 2 . It may be seen from figure 9 presented in our JHEP11(2018)186 previous work [1]. Similarly, a correction of the fourth power does not give a significant contribution to the square of the energy for the case s z = 0. Therefore, we obtain the dipole magnetic polarizability for the spin projection s z = 0 from the fit of lattice data by the following relation at eB ∈ [0, 1.2] GeV 2 , where eB is the magnetic field in GeV 2 , β m is the dipole magnetic polarizability and fit parameter, m is the fit parameter also. The lattice results together with the fitting curves are shown in figure 2 which shows the energy squared increasing with the magnetic field value. At eB ∼ 0.2 ÷ 0.3 GeV 2 we observe a hump which leads to increase of the errors in determination of β m (s z = 0) value. It can be a result of lattice spacing and lattice volume effects or have some physical explanation. We cannot perform a rigorous analysis due to high errors of the calculations, but we note that this hump is absent for the lattice with smaller lattice spacing a = 0.095 fm. Therefore it is more probably a lattice spacing artefact. The values of the β m with the values of χ 2 /n d.o.f. and lattice parameters are shown in table 2.
The behaviour of the energy squared for the case qs z = +1 (which corresponds to ρ − at s z = −1 and ρ + at s z = +1) can be described by the dependency  In figure 4 we represent the energy squared for different meson spin projections on the field axis for the lattice volume 18 4 , the lattice spacing a = 0.115 fm and the pion mass equal to 541 MeV. The energy errors for the case qs z = −1 are sufficiently high. For the case qs z = −1 the fit was using the formula To estimate the contribution of the magnetic dipole polarizability to the lepton asymmetry it is needed to know the dipole magnetic polarizability for the s z = +1 and s z = −1     cases. However, due to big statistical errors the magnetic dipole polarizability cannot be obtained from the energy dependence at s z = +1 if we consider ρ − or from s z = −1 if we consider ρ + . Nevertheless, the parity conservation demands the equality of the magnetic dipole polarizabilities for s z = +1 and s z = −1. Then it follows from (5.3) and (5.4) In order to make sure that the relation (5.5) is satisfied for our data we represent the value of (E 2 qsz=−1 − E 2 qsz=+1 )/2 versus the magnetic field value in figure 5. This quantity increases linearly with the magnetic field. The values of the g-factor obtained from these fits are equal to 2. effective mass plateau is very noisy for the qs z = −1. We have determined the g-factor from the lowest energy sub-level in our previous work [1].

Magnetic polarizability of the ρ 0 meson
We have discussed the magnetic polarizabilities of the neutral ρ mesons previously in [11], where we considered the toy model with one type of quarks. In an external magnetic field the u-and d-quarks couple differently to the magnetic field. It has to be taken into account when we calculate the physical observables. We repeat the analysis represented in [11] with the difference that we find the energies from the correlation function (3.3) and increase the statistics.
In the relativistic case the energy of the neutral ρ meson with spin projection s z = 0 is described by the following dependency where β h2 m , β h4 m and β h6 m are the various magnetic hyperpolarizabilities of higher orders, m is the mass of the meson at zero field.
In figure 6 we represent the energy squared of the ρ 0 meson with s z = 0 versus the field squared for various lattices and pion masses at (eB) 2 ∈ [0 : 0.5] GeV 4 . The lattice data are depicted by points. We observe the energy decrease rapidly for all the lattice data. It also strongly depends on the lattice spacing, the lattice volume, and the pion mass. The lines are the fits of these data obtained with the use of formula (6.1) when we also include terms ∼ (eB) 10 Table 4. The value of the magnetic dipole polarizability β m and the magnetic hyperpolarizability β 2h m for the ρ 0 with spin projection s z = 0 are shown for the various lattice volumes V , lattice spacings a and pion masses m π . The degree of polynomial n, field range used for the fitting and χ 2 /d.o.f values are represented in columns sixth to eighth correspondingly. extract the magnetic polarizability, because the quantization condition imposes a limitation on the minimal field value. We do not perform an extrapolation to the chiral limit since we are interested only in the qualitative predictions at this stage of investigations.
In table 4 one can find the magnetic polarizability β m and hyperpolarizability β 2h m obtained from the fits. The lattice volume V , the lattice spacing a, the pion mass m π , the interval of fields selected for the fitting procedure and χ 2 /n.d.o.f. are also shown. The results agree with each other within the errors. At eB ∈ [0 : 1.2] GeV 2 for the spin projection |s z | = 1 on the field axis the energy squared of the neutral vector meson can be described by the following relation:

Tensor magnetic polarizability
In the previous sections we have found that the energy of the ρ 0 meson with s z = ±1 increases versus the magnetic field value, while the energy of the ρ 0 meson with s z = 0 diminishes quickly versus the magnetic field value. For the ρ ± the energy decreases for the case qs z = +1 and increases for the qs z = 0 and qs z = −1 cases.

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Such energy behaviour has some physical consequences. The small energy is more profitable than the high energy, so the longitudinal polarization of the ρ 0 meson corresponding to s z = 0 has to dominate in the collisions. Therefore, in the non-central heavy-ion collision the magnetic field favours longitudinal polarization of the ρ 0 mesons.
The dilepton asymmetries in non-central heavy ion collisions depend on the energy behaviour of the vector mesons. According to the vector dominance principle the vector mesons can directly convert to virtual photons. In turn, the electromagnetic decay of virtual photons is one of the main sources of dilepton production in heavy-ion collisions. When dileptons are produced in non-central heavy-ion collisions, their anisotropy depends on the response of the spin structure of intermediate resonances, such as ρ 0 to the magnetic field of the collision. Therefore, it is of particular interest to identify and distinguish between various sources of dileptons emitted from non-central heavy-ion collisions.
The shape of the dilepton distribution is characterized by the following differential cross section: where M 2 = (p 1 + p 2 ) 2 is the energy of the lepton pair in their rest frame, p 1 and p 2 are the four-momenta of the leptons, θ is the angle between the momenta of the virtual photon and the lepton. The asymmetry coefficient B is defined by the polarization of the virtual photons produced in the collisions: where the γ ⊥, are the contributions of the transverse and longitudinal polarizations of the virtual intermediate photon.
Our lattice calculations make possible to get the estimation of the asymmetry factor for such processes. For the vector particle in Cartesian basis the polarization tensor has the following form If w sz=+1 , w sz=−1 and w sz=0 are the probabilities that the ρ meson has a spin projection on the field direction equal to +1, −1 and 0 correspondingly, then the value of the component P 33 can be represented in terms of these probabilities in the following form: where N sz=+1 , N sz=−1 and N sz=0 are the numbers of particles with different spin projections.
As w sz=+1 + w sz=−1 + w sz=0 = 1, therefore, P 33 = 1 − 3w sz=0 and −2 ≤ P 33 ≤ 1. The tensor polarizability describes the effect of the magnetic field for the spin states of the ρ meson, in turn, the spin states and tensor polarization is revealed in its decay to lepton pair, see [24]. In a strong magnetic field the spin of the particle tends to align along the field direction, but the non-zero temperature leads to the spin-flipping.  Table 7. The tensor polarizability β t of the ρ ± is represented for various lattices and pion masses.
The differential cross section for the decay of ρ meson to the lepton pair may be written as dσ Comparing with (7.1) one can see that For the transversely polarized ρ meson B = 1 and for the longitudinally polarized B = −1.
We also introduce the tensor polarizability which is the measure of the magnetic field effect on a vector meson, in particular for high magnetic fields and temperature P ∼ β t . We calculate β t on the lattice taking into account the equality β sz=+1 = β sz=−1 . The results are presented in table 6 for the neutral ρ-meson and in table 7 for the charged ρ-meson. The large negative values of β t suggest the dominating longitudinal polarization of the ρ 0 -meson. The dileptons are mainly emitted in the directions perpendicular to the magnetic field axis. This is a convincing result, as we clearly see from figure 6 and 7,that the energy of the state with s z = 0 decreases, and the energy of |s z | = 1 increases.
It was found previously that for soft dileptons the longitudinal polarization also dominates [34]. This result was obtained by comparing the formation of soft dileptons with a nonzero component of the conductivity of the strongly interacting matter, parallel to the external magnetic field [35].

JHEP11(2018)186 8 Conclusion
In this paper the calculation of the magnetic dipole and tensor polarizabilities have been presented for the charged and neutral ρ mesons on the lattice volume. We perform a thorough analysis of the behaviour of the effective mass plateau depending on the number of points used for the fitting by hyperbolic cosine function.
In section 5 the magnetic dipole polarizability and g-factor for the charged mesons have been represented. We include the additional sets of data into consideration and increase statistics with the lattice spacing a = 0.105 fm and volume 18 4 . This allows one to obtain the more statistically significant values of the magnetic dipole polarizabilities for the spin projection s z = 0, see table 4. In contrast to the previous results [1], we have calculated the dipole magnetic polarizability for the case qs z = 1 from the 3-parametric fit (5.3), where the g-factor is a free parameter of the fit. Obviously, we could find the g-factor values at smaller field interval and use these values for the β m determination, but the purpose of this work was to obtain the qualitative predictions.
In section 6 the dipole magnetic polarizability have been extracted for the case of the neutral ρ meson. The magnetic dipole polarizability was calculated, taking into account that the u and d-quarks couple differently to the magnetic field. In [11] the magnetic dipole polarizability of ρ 0 was calculated in the toy model with only one type of quark. Section 7 is devoted to the discussion of the polarization of the dileptons which result from the decays of ρ mesons. We have found that the longitudinal polarization of the ρ 0 mesons dominates in the collisions, because the low energy is more preferential than high energy. Therefore the dileptons occurring due to decays of the ρ 0 mesons will be emitted perpendicular to the direction of the magnetic field. This result reinforces the previous results obtained in [35], i.e. the nonzero conductivity of the quark-hadronic matter in a strong magnetic field. We introduce new characteristics of the meson magnetic properties -the tensor palarizability. This quantity has been suggested to be related to the coefficient of asymmetry in the differential cross section for the dilepton production.