Excitonic pairing of two-dimensional Dirac fermions near the antiferromagnetic quantum critical point

Excitonic pairing of two-dimensional Dirac fermions near the antiferromagnetic quantum critical point

Hai-Xiao Xiao Department of Modern Physics, University of Science and Technology of China, Hefei, Anhui 230026, P. R. China    Jing-Rong Wang Anhui Province Key Laboratory of Condensed Matter Physics at Extreme Conditions, High Magnetic Field Laboratory of the Chinese Academy of Science, Hefei, Anhui 230031, P. R. China    Zheng-Wei Wu Department of Modern Physics, University of Science and Technology of China, Hefei, Anhui 230026, P. R. China    Guo-Zhu Liu gzliu@ustc.edu.cn Department of Modern Physics, University of Science and Technology of China, Hefei, Anhui 230026, P. R. China
Abstract

Two-dimensional Dirac fermions are subjected to two types of interaction, namely the long-range Coulomb interaction and the short-range on-site interaction. The former induces excitonic pairing if its strength is larger than some critical value , whereas the latter drives an antiferromagnetic Mott transition when its strength exceeds a threshold . Here, we study the impact of the interplay of these two interactions on the fate of excitonic pairing by using the Dyson-Schwinger equation approach. We find that the value of is slightly increased by weak on-site interaction. As grows to approach , the quantum fluctuation of antiferromagnetic order parameter becomes important and interacts with Dirac fermions via the Yukawa coupling. After treating the Coulomb interaction and Yukawa coupling on equal footing, we show that increases substantially as . Therefore, excitonic pairing is strongly suppressed near the antiferromagnetic quantum critical point. We obtain a global phase diagram on the - plane, and illustrate that the excitonic insulating and antiferromagnetic phases are separated by the gapless semimetal phase. These results provide a possible explanation of the discrepancy between recent theoretical progress on excitonic gap generation and existing experiments in suspended graphene.

I Introduction

Two-dimensional (2D) massless Dirac fermions are the low-energy excitations of a number of condensed matter systems. Examples include -wave high- cuprate superconductors LeeRMP (); Orenstein (), graphene Novoselov04 (); Novoselov05 (); CastroNeto (); DasSarma (); Kotov (), surface of three-dimensional (3D) topological insulators topo (), and organic conductor -(BEDT-TTF)I Hirata16 (). While the single particle properties of Dirac fermion systems have already been extensively studied, the strong correlation effects are still not well understood. Ordinary metals are known to be robust against repulsive interactions Shankar94 (), which renders the validity of Fermi liquid theory. In contrast, the repulsive interactions are much more important in 2D Dirac fermion systems, and may lead to several possible phase-transition instabilities CastroNeto (); DasSarma (); Kotov (). Generically, there are two types of repulsive interactions, namely long-range Coulomb interaction and Hubbard-like on-site interaction. The former is spin blinded, whereas the latter acts on two electrons with different spins.

When the strength parameter of on-site repulsive interaction is greater than a critical value , there is a quantum phase transition from gapless semimetal (SM) to antiferromagnetic (AFM) Mott insulator Herbut06 (). The SM-AFM quantum critical point (QCP) falls in the university class of Gross-Neveu-Yukawa model Herbut06 (). Apart from SM-AFM transition, Sato et al. Sato17 () studied the transition between SM and Kekulé valence-bond solid caused by on-site interaction. When other sorts of repulsion are considered, SM materials could exhibits even richer phase-transition structures Raghu08 (); Weeks10 (); Grushin13 (); Daghofer14 (); Sato17 (); Zeng18 (); Tang18 (); Buividovich18 (). For instance, Raghu et al. Raghu08 () investigated the cooperative effects of nearest-neighboring and next-neighboring repulsions within the mean-field approximation, and found a number of insulating phases, including charge density wave (CDW), AFM, and topological Mott phases that display quantum anomalous Hall (QAH) and quantum spin Hall (QSH) effects, although subsequent studies revealed that the topological Mott phases can be destroyed by fluctuations Daghofer14 ().

In case the Fermi level is located exactly at the band-touching point, the long-range Coulomb interaction is poorly screened due to the vanishing of density of states (DOS). If the Coulomb interaction is weak, the system remains gapless, but the fermion velocity is substantially renormalized Kotov (); Geim11 (). When the Coulomb interaction strength parameter exceeds a critical value , a finite energy gap is dynamically generated via the formation of excitonic-type particle-hole pairs Khveshchenko01 (); Gorbar02 (); Khveshchenko04 (); Liu09 (); Khveshchenko09 (); Gamayun09 (); Sabio10 (); Gamayun10 (); WangLiu12 (); Popovici13 (); Gonzalez15 (); Carrington16 (); Carrington18 (); Xiao17 (); Drut09A (); Drut09B (); Drut09C (); Armour10 (); Armour11 (); Buividovich12 (); Ulybyshev13 (); Smith14 (); Juan12 (); Kotikov16 (); Tupitsyn17 (). This then turns the originally gapless SM into a gapped excitonic insulator (EI).

In previous works, the Coulomb interaction and the on-site interaction were usually investigated separately. Their interplay can give rise to some salient properties, especially in the strong coupling regimes. Interesting progress has recently been made towards more detailed knowledge of this interplay. Tang et al. Tang18 () studied the influence of long-range Coulomb and on-site interactions on the ground-state properties of 2D Dirac fermion systems by combining the non-perturbative quantum Monte Carlo (QMC) simulation and the renormalization group (RG) technique. Their works Tang18 () reproduced the previously discovered logrithmic velocity renormalization and also the SM-AFM transition at some critical value . They further showed that increases as grows, which indicates that the Coulomb interaction disfavors AFM transition. These results are summarized in the phase diagram given by Figure 1 of Ref. Tang18 ().

The results of Ref. Tang18 (), and also those of Ref. Buividovich18 (), are restricted to the region of weak Coulomb interaction. The region of strong Coulomb interaction appears to be inaccessible to the numerical methods developed in Ref. Tang18 (); Buividovich18 (). As aforementioned, strong Coulomb interaction is able to induce excitonic gap generation. This problem has attracted broad interest in the past two decades. Extensive theoretical efforts have been devoted to examining whether the SM-EI transition takes place in graphene. In Refs. Tang18 (); Buividovich18 (), the influence of on-site interaction on SM-EI transition has not been addressed. Moreover, it remains unclear how the SM-EI transition is affected by the SM-AFM quantum criticality.

Figure 1: The global phase diagram of 2D Dirac fermion system on the plane spanned by Coulomb interaction parameter and on-site interaction parameter . The critical line of is taken from Ref. Tang18 (). The solid part of the EI critical line is plotted based on our DS equation results, and the dashed part of this line is plotted based on extrapolation.

In this paper, we study the excitonic pairing of 2D Dirac fermions by considering both the Coulomb and on-site interactions. In particular, we investigate the impact of on-site interaction on the fate of excitonic pairing. For small values of , the Coulomb interaction and on-site interaction need to be treated on equal footing. When grows, the AFM correlation is gradually enhanced. As , the system approaches to the AFM QCP and the quantum fluctuation of AFM order parameter is coupled strongly to Dirac fermions. To examine the influence of AFM quantum criticality on excitonic pairing, we need to treat the interplay between the Coulomb interaction and the Yukawa coupling.

The non-perturbative Dyson-Schwinger (DS) equation approach will be employed to compute the excitonic gap and to determine . In our calculations, the series expansion is controlled by the factor , where is the spin degeneracy of Dirac fermion. Thus the Coulomb interaction parameter can take any value. This will allow us to access the strong Coulomb interaction regime. The Yukawa coupling between the AFM fluctuation and the Dirac fermion is also handled by the expansion. However, the on-site interaction is spin distinguished, to be explained below, and expansion becomes invalid in this case. We will only consider weak on-site interaction and perform weak coupling expansion.

After taking into account the impact of weak on-site interaction, the critical value for EI transition is only slightly increased. At the AFM QCP (), increases dramatically as the Yukawa coupling constant grows. Apparently, the excitonic gap generation is significantly suppressed by the quantum fluctuation of AFM order parameter. As decreases from , the system departs from the QCP and the suppression of excitonic pairing caused by the AFM fluctuation is gradually weakened. Combining these results with those reported in Ref. Tang18 (), we obtain a schematic global phase diagram on the - plane, shown in Fig. 1. It seems that the EI phase cannot be directly converted into the AFM Mott phase: they are separated by an intermediate SM phase.

A direct application of our results is that it offers a possible explanation of the discrepancy between recent theoretical finding and existing experiments in graphene. It is known that takes its maximal value when graphene is suspended in vacuum. The zero-temperature ground state of suspended graphene should be an insulator if . The values of obtained by employing different approximations of DS equation are quite different. In a recent work, Carrington et al. Carrington18 () has gong beyond many of the previously used approximations, and found that , slightly below . This result suggests that suspendend graphene may be an insulator at zero temperature. However, this is apparently at odds with experiments Geim11 (). According to the analysis of Refs. Wehling11 (), graphene seems to be close to the AFM QCP, thus the impact of AFM quantum criticality on needs to be seriously taken into account. Our results show that the proximity to the AFM QCP significantly increases the critical value , which makes SM-EI transition very unlikely to happen in realistic graphene.

The rest of the paper is organized as follows. In Sec. II, we present the DS equation for dynamical excitonic gap. The gap equation is solved and analyzed in Sec. III, and the physical application of the result is discussed in Sec. IV. The results are summarized in Sec. V.

Ii Dyson-Schwinger gap equation

Free 2D Dirac fermion system is described by the Lagrangian in Minkowski space

(1)

where is a four-component spinor field and . The index sums from to , with being the spin degeneracy of Dirac fermion. The gamma matrices are defined via the standard Pauli matrices as , which satisfy the Clifford algebra. The fermion velocity is taken be a constant.

We will consider three different sorts of interactions, including the long-range Coulomb interaction, the spinful on-site interaction, as well as the Yukawa coupling between Dirac fermions and AFM quantum fluctuation. If the system is far from the AFM QCP, we only need to study the first two interactions. But when the system is sufficiently close to the AFM QCP, the interplay of Coulomb interaction and Yukawa coupling should be carefully investigated. Below we present the effective field theories for these three interactions in order.

ii.1 Pure Coulomb interaction

The pure Coulomb interaction can be modeled by the following Lagrangian

(2)

where is an auxiliary scalar field introduced to represent Coulomb interaction. It is easy to verify that the Lagrangian respects the continuous chiral symmetry .

Figure 2: Feynman diagram of and . The difference between two diagrams lies in the expression of the vertices.

The pure Coulomb interaction has already been widely studied Khveshchenko01 (); Gorbar02 (); Khveshchenko04 (); Liu09 (); Khveshchenko09 (); Gamayun09 (); Gamayun10 (); WangLiu12 (); Carrington16 (); Carrington18 (); Xiao17 () previously. Here we only briefly summarize the main results for latter usage. As mentioned in Sec. I, the Coulomb interaction will be studied by employing the expansion. In this paper, we will retain the leading order contribution of expansion, and ignore the contribution of wave function renormalizations. The validity of this approximation will be discussed later. The free propagator of Dirac fermions is

(3)

Interaction corrections alters this propagator into

(4)

where is fermion self-energy function. Once acquires a finite value due to the Coulomb interaction, an excitonic mass gap is generated and the gapless SM is converted into a fully gapped EI. In order to examine whether an excitonic gap is generated, we write down the following DS equation

(5)

where and . Here, the effective Coulomb interaction is given by

(6)

where is the polarization function and

(7)

is the bare Coulomb interaction, with being the dielectric constant. To the leading order of expansion, the Feynman diagram for is shown in Fig.2. At the random phase approximation (RPA) level, the one-loop is calculated as follows Khveshchenko01 ()

(8)

After preforming the Wick rotation(), we get the following DS gap equation in Euclidean space Khveshchenko01 ()

(9)

where a new parameter is defined to measure the effective interaction strength. For a given flavor , the above gap equation has a nontrivial solution, i.e., , only when . The QCP between SM and EI phases is located at . If the value of is fixed, a nonzero gap could be generated only when .

ii.2 Weak on-site interaction

As showed by Herbut and his collaborators Herbut06 (); Herbut09 (), the generic on-site interaction is complex and can be decomposed into eight independent four-fermion coupling terms. Here, following Ref. Tang18 (), we only consider the spin-distinguished interaction term

(10)

which is responsible for the emergence of AFM Mott insulating phase. In Ref. Tang18 (), this is referred to as spinful Gross-Neveu (GN) interaction. It is also called chiral Heisenberg GN interaction Gracey18 (). According to Ref. Herbut06 (), is related to through the identity .

Upon expanding the quadratic term appearing in , we get two sorts of four-fermion couplings

(11)

For a given spin , the coupling amounts to the GN interaction with flavor . Such a coupling term cannot be treated by means of expansion. The coupling constant has the dimension of inverse mass. It is convenient to define a dimensionless parameter , where the momentum cutoff is connected to the lattice spacing via the relation . In the following, we will choose to carry out series expansion in powers of . This method is invalid in the strong coupling regime. Tang et al. Tang18 () have numerically investigated the strong coupling regime by means of quantum MC simulation and found that the system enters into AFM Mott insulating phase once becomes sufficiently large.

Figure 3: Diagrams of leading () and sub-leading () order contributions to the GN interaction kernel. Blue solid line stands for fermions with spin , and red solid line for spin .

We first ignore the Coulomb interaction and examine whether or not the pure GN interaction leads to dynamical generation of excitonic gap. According to the analysis of Ref. Dorey90 (), the DS equation can be formally written as

(12)

where is the four-fermion interaction kernel. can be obtained from the sum of all the two-particle irreducible vacuum diagrams in the full fermion propagators Dorey90 (), represented by . is connected to the kernel in the following way

(13)

In this paper, we will retain both the leading order and sub-leading order corrections. The corresponding Feynman diagrams are presented in Fig. 3.

The leading order contributions to are

(14)

The sub-leading order contributions are

(15)
(16)

where and , and we define

(17)

which is independent of spin directions. After doing simple calculations, we find that . From Fig. 3, we see that the first two orders of corrections satisfy the relation Dorey90 () for both and . Therefore, the DS equation for fermion self-energy takes the form

(18)

In the small region, we ignore the fermion damping and velocity renormalization, thus the fermion self-energy can be identified as the excitonic mass gap. Upon making Wick rotation, we derive the following DS gap equation

(19)

The leading order correction to dynamical gap generation has been previously analyzed in Ref. Kaveh05 (). Notice there is a sign difference in the definition of . In Ref. Kaveh05 (), a finite gap is generated only when (in the limit of ); in our case the critical value becomes . In this work we only consider negative , thus the GN interaction cannot induce excitonic pairing by itself. However, the GN interaction might affect the fate of excitonic pairing induced by the Coulomb interaction. This will be studied in Sec. III.1.

ii.3 Yukawa coupling near AFM QCP

When the strength of spinful GN interaction increases, the AFM correlation is enhanced. The gapless Dirac SM would become an AFM Mott insulator once exceeds some critical value , which defines a zero temperature AFM QCP. As revealed by Tang et al. Tang18 (), appears to be an increasing function of in the region of weak Coulomb interaction. Previous studies on such an AFM quantum criticality Herbut06 (); Herbut09 () revealed that the Yukawa coupling between Dirac fermions and the AFM quantum critical fluctuation, described by scalar field , determines the low-energy properties of the AFM quantum critical phenomena if Coulomb interaction is ignored. Here, we are particularly interested in whether the excitonic pairing is suppressed or promoted near the AFM QCP.

To describe the AFM fluctuation, we add to the following additional terms

(20)

where is the strength parameter for Yukawa coupling and is fermion spin. The AFM order parameter Herbut06 (); Tang18 () is given by . The scalar field stands for the quantum fluctuation around this mean value. The boson mass can be identified as the tuning parameter for SM-AFM transition, and at the QCP . Here, we only consider the SM side of the QCP, and thus suppose . To facilitate analytical calculations, we introduce two new coupling constants for two spin components: . It is worth mentioning that have the same dimension as .

Figure 4: Feynman diagram of fermion self-energy.

Once is introduced, the continual chiral symmetry is explicitly broken. Nevertheless, the total action still preserves a discrete chiral symmetry , so long as the scalar field transforms simultaneously in the following way: . If a finite gap is generated, the above discrete chiral symmetry will be broken.

The Feynman diagrams of the fermion self-energy are shown in Fig. 4, where stands for the dressed Coulomb interaction function and for the dressed propagator of the field. To the leading order of expansion, we need to consider the following DS equation

where and .

The free propagator of is . Similar to the Coulomb interaction, this free propagator is also renormalized by collective excitations. Including this effect leads to a dressed bosonic propagator

(22)

in which the polarization function , whose diagram is presented in Fig. 2, is given by

(23)

to the leading order of expansion. According to the detailed derivation shown in Appendix. A, we find

(24)

After performing a series of analytical calculations, we arrive at the following gap equation

(25)

where the Wick rotation has been performed. There is a minus sign in the contribution due to the Yukawa coupling. Two important facts can be deduced. First, the Yukawa coupling tends to suppress excitonic pairing. Second, the Yukawa coupling by itself is not able to trigger excitonic pairing.

Figure 5: The -dependence of zero-momentum excitonic gap at and .

Iii Numerical results

In this section, we solve the DS equations numerically and analyze the physical implications of the solutions. We will first consider the case of weak GN interaction and then the vicinity of AFM QCP. Our aim is to determine their influence on the value of .

iii.1 Interplay of Coulomb and GN interactions

To examine the interplay between the long-range Coulomb and short-range GN interactions, we combine Eq. 9 and Eq. 19, and then solve the total gap equation self-consistently for different values of at and (the physical value of in suspended graphene). The energy cutoff is chosen as .

Figure 6: The -dependence of zero-momentum gap for different values of at .

To simplify numerical evaluation, it is useful to first adopt the commonly used instantaneous approximation Khveshchenko01 (), which assumes that the fermion gap and Coulomb interaction are independent of energy. The impact of energy dependence will be examined later. Under this approximation, the total gap equation has the form

(26)

After solving this equation, we present the numerical results in Fig. 5, where is defined as the value of fermion gap at zero energy and zero momentum. As grows, decreases considerably. This implies that weak GN interaction tends to suppress excitonic gap. The -dependence of is shown in Fig. 6. We observe that, as GN interaction is becoming stronger, the value of is slightly increased. In particular, for , .

The instantaneous approximation has been previously used in the DS study of excitonic gap generation Khveshchenko01 (). More refined works Carrington18 () have confirmed that the value of obtained under this approximation is actually not far from the one obtained by incorporating higher order corrections. In this regard, the instantaneous approximation leads to qualitatively reliable conclusion. We have solved the gap equation after incorporating the energy dependence of gap function and Coulomb interaction, and found that the qualitative conclusions are the same but the concrete values of and are more or less changed.

iii.2 Interplay of Coulomb interaction and Yukawa coupling

We now consider the interplay of Coulomb interaction and Yukawa coupling. The corresponding DS gap equation is given by Eq. 25. To obtain the numerical results, a renormalization procedure has to be taken, in which the dimension of all parameters will be eliminated by dividing either or . The parameters appeals blow are renormalized without explicitly statement. To get a rapid glimpse of the main results, we first neglect the energy dependence of fermion self-energy and interaction functions, which leads to

(27)
(28)
(29)

Now DS gap equation is simplified to

(30)
Figure 7: The -dependence of for different values of at . Clearly, is an increasing function of .
Figure 8: The critical line of SM-EI transition on the - plane. Here the Coulomb interaction parameter is fixed at .

We have solved this equation numerically, and now show in Fig. 7 the -dependence of excitonic gap obtained at zero momenta, namely , for different values of . If the AFM QCP is entirely ignored, corresponding to , the critical value . If takes a very small value , is increased to . For and , we find that and , respectively. Therefore, the excitonic gap generation can be significantly suppressed at the AFM QCP.

Further, we study how changes the critical fermion flavor . We fix at , and solve Eq. (34) to obtain the relation between and , with results presented in Fig. 8. For very small values of , . For , is reduced below . For a Dirac fermion with physical flavor , excitonic pairing is completely forbidden in the presence of sufficiently strong Yukawa coupling.

Figure 9: The -dependence of at a number of values of . Here the fermion flavor is .

The dependence of on at fixed flavor is shown in Fig. 9. At the AFM QCP with , increases rapidly as grows, and finally goes to infinity at sufficiently large . This is another signature that AFM quantum criticality disfavors excitonic gap generation. As increases, the system moves away from the AFM QCP into the SM region. In this process, the quantum fluctuation of AFM order parameter is weakened, and the suppressing effect of excitonic pairing becomes progressively unimportant.

In Ref. Tang18 (), the authors revealed that Coulomb interaction tends to increase . Here we have showed that AFM quantum fluctuation can suppress excitonic pairing. There seems to be a repulsion between the excitonic pairing and the AFM ordering. Based on these results, we plot a schematic phase diagram on the - plane in Fig. 1. The critical line of goes rightwards as increases Tang18 (), whereas the critical line of goes upwards as from the left side. A previous RG study Herbut06 () predicted that the Dirac fermion system may undergo a first-order transition from EI to AFM Mott insulator. Our results indicate that such a direct transition does occur, and that the excitonic insulating phase and AFM Mott insulating phase are actually separated by an intermediate gapless SM phase.

We have also numerically solved Eq. (30) after including the retardation effects ( at ) and reached the same conclusion that the quantum AFM criticality suppresses excitonic gap generation. Therefore, the schematic phase diagram presented in Fig. 1 is still qualitatively correct after taking the energy dependence into account.

Iv Application of the results

Determination of the precise value of proves to be a highly nontrivial challenge. In QED and QED, the fermion propagator, the gauge boson propagator, and the fermion-boson vertex function form a closed set of integral equations Roberts94 (). This result is valid in our case because the Coulomb interaction can be effective described by the interaction between the Dirac fermion and the temporal component of U(1) gauge boson. The full fermion propagator has the generic form

where and are the wave function renormalizations and is the fermion gap function. The full boson propagator is given by Eq. 6, and the vertex function can be represented by . The DS equations contain all the information caused by interactions. Once the complete expression for the vertex function is derived, the full fermion and boson propagators can be determined. In practice, it is not possible to obtain the exact solutions of DS equations, and one always needs to introduce certain approximations (truncations) to replace full propagators and/or full vertex function. There are two commonly used vertex functions: the bare vertex and the Ball-Chiu BallChiu () vertex.

Extensive DS equation studies of excitonic pairing in graphene have showed that the value of is very sensitive to the specific approximation. To demonstrate this, we list in Table I a number of representative values of obtained by employing various approximations. If one assumes and ignores vertex correction, in the instantaneous approximation and after including the energy dependence. Two of the authors incorporated and , utilized the first term of Ball-Chiu vertex, and adopted the RPA expression of polarization , and found WangLiu12 () . It was pointed out in Ref. WangLiu12 () that could be considerably decreased if the feedback of excitonic gap on is included. Recently, Carrington et al. Carrington18 () have carried out carefully DS equation calculations after taken into account and , the first term of Ball-Chiu vertex, and also the feedback of , , and on , and obtained . It is surprising that the value obtained in the present paper by using the very crude instantaneous approximation is actually quite close to the above result. Moreover, the obtained by Carrington et al. Carrington18 () is smaller than the physical value of suspended graphene. In the light of this result, one might have to conclude that clean, undoped suspended graphene is an EI at low temperatures.

Reference
1.9 current paper
0.92 Gamayun09 ()
0.7 current paper
3.2 WangLiu12 ()
2.9 Carrington16 ()
1.99 Carrington18 ()
2.06 Carrington18 ()
Table 1: DS equation results for the critical value at the flavor . , , , and are defined in the context. stands for the Ball-Chiu vertex correction. is the RPA-level polarization given by Eq. (8), and represents the polarization function obtained from self-consistent DS equation calculations. The symbol refers to the instantaneous approximation, and indicates that the energy dependence is taken into account. The corresponding function is neglected if the space is left blank.

Ellias et al. Geim11 () has measured the cyclotron mass in suspended graphene and found no evidence of finite gap at rather low energies (). This finding was further supported by the measurements of Mayorov et al. Mayorov12 (). How can one reconcile the recent theoretical result of Carrington et al. Carrington18 () and these experiments?

Here we propose that the seeming discrepancy can be explained by noting the fact that graphene is not far from the AFM QCP. Wehling et al. Wehling11 () has calculated the on-site interaction parameter by using three different approaches. The critical value needed to trigger AFM Mott transition seems to be only slightly larger than the physical Tang18 (), which implies that realistic graphene is close to the AFM QCP Tang18 (). Apparently, the AFM quantum fluctuation is important in graphene and should be seriously considered in the study of the EI transition. As revealed in our calculations, AFM quantum fluctuation can strongly suppress excitonic pairing by increasing the value of . Therefore, we conclude that the gapless SM state of suspended graphene is actually quite robust.

V Summary and Discussion

In summary, we have investigated the non-perturbative effect of dynamical excitonic gap generation in a 2D Dirac fermion system. The Dirac fermions are subjected to two types of interaction, namely the long-range Coulomb interaction and the short-range on-site interaction. The former interaction can trigger excitonic pairing, whereas the latter leads to AFM quantum phase transition in the strong coupling regime. The DS equation approach is employed to study the influence of GN-type on-site interaction on the fate of SM-EI transition. We first have showed that the GN interaction only leads to weak suppression of excitonic gap generation. As the system approaches to the AFM QCP, the dynamics of Dirac fermions is strongly influenced by the quantum critical fluctuation of AFM order parameter. We have demonstrated that excitonic gap generation is suppressed by AFM quantum fluctuation. Such a suppression effect is most significant at the AFM QCP, but gradually diminishes when the system moves away from the QCP. If 2D Dirac fermion system is close to the AFM QCP, as what happens in graphene, it would be very difficult to realize excitonic pairing.

Based on these results, we provide supplementary new information to the global phase diagram reported in Ref. Tang18 (). On the phase diagram, the EI phase is not neighboring to the AFM phase, but is separated from the AFM phase by an intermediate SM phase, as illustrated schematically in Fig. 11. This conclusion is different from the one previously reported in Ref. Herbut06 (). Our results indicates that it is hardly possible to transform 2D Dirac fermion system from an EI phase directly to AFM Mott phase. The reason is that the quantum critical AFM fluctuation prevents excitonic pairing.

When both and take large values, the Dirac fermion system could either be a AFM Mott insulator or enters into a CDW phase due to excitonic pairing, or remain as a semimetal. To determine the quantitatively more precise phase diagram in such a highly interacting regime, it is necessary to investigate the mutual influence between strong Coulomb interaction and strong on-site interaction in a more self-consistent manner, which will be carried out in future works.

Acknowledgements.
The authors acknowledge the financial support by the National Natural Science Foundation of China under Grants 11847234, 11574285, and 11504379.

Appendix A Calculation of the polarization

We now provide the calculational details of the polarization function for the dressed propagator of bosonic AFM fluctuation. To the leading order of expansion, this polarization is defined as

(31)

where is a constant mass of Dirac fermion. Making the replacements and , we re-write it in the form

(32)

Making use of the Feynman integral

(33)

we proceed as follows

(34)

Define and , we further get

Introducing leads to

Since

(36)

we find that

After carrying out a series of calculations, we eventually obtain

(37)

where is an UV cutoff. In the massless limit, i.e., , we have

(38)

After Wick rotation(), we can have the polarization function in Euclidean space

(39)

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