Research Article  Open Access
Towards Reviving Electroweak Baryogenesis with a Fourth Generation
Abstract
Electroweak baryogenesis is an attractive scenario for explaining the baryon asymmetry of the universe. However, it does not work within the standard model due to two reasons: (1) the strength of CP violation from the KobayashiMaskawa mechanism with three generations is too small; (2) the electroweak phase transition is not first order for the experimentally allowed Higgs boson mass. We discuss possibilities to solve these problems by introducing a fourth generation of fermions and how electroweak baryogenesis might be revived. We also discuss briefly the recent observation of a Higgslike boson with mass around 125 GeV, which puts the fourth generation in a difficult situation, and the possible way out.
1. Introduction
The origin of the baryon asymmetry of the universe (BAU) is not only a big mystery in particle physics and cosmology, but it is a core problem related to our very existence. The observational evidence is very compelling. There is no indication for any macroscopic objects made from antiparticles. The antiparticles observed in cosmic rays are thought to be of secondary origin. Thus, it is accepted that the universe contains negligible amount of antibaryons, as compared to the baryons that constitute usual matter (including ourselves!), or . The standard big bang cosmology requires the baryontoentropy ratio of the universe to be [1] If one does not take the view that this is merely an initial condition for the expanding universe, then the challenge is not so much the dominance of radiation, but that whether there is any matter left from the primordial matterantimatter annihilation.
Many scenarios have been attempted to explain the origins of the minute amount of leftover matter based on a dynamical mechanism (baryogenesis). A common basis for such mechanisms is provided by the three Sakharov conditions [2, 3], which consist of (i) baryon number () violation, (ii) and CP violation, and (iii) departure from equilibrium. In order to produce the BAU, these three conditions have to be satisfied simultaneously at some stage in the early universe.
Among many proposals, electroweak baryogenesis (EWBG) [4] is one of the wellmotivated and appealing mechanisms to explain BAU, especially since its ingredients can be possibly probed by the Large Hadron Collider (LHC). This mechanism could operate during the electroweak phase transition (EWPT), occurring when the temperature of the universe is around GeV, and it is a possible baryogenesis mechanism within the standard model (SM) of particle physics. One should recall the truly remarkable fact that the SM carries all the necessary ingredients for the Sakharov conditions.(1) is violated due to the chiral anomaly induced by the gauge interaction. violating processes are nonperturbative phenomena mediated by topologically nontrivial SU(2) gauge field configurations. Although the instantonmediated violation at zero temperature is highly suppressed, the rate of violation at finite temperature is not negligible via the socalled sphaleron transition, especially when the temperature is around or above . (2) is violated by the structure of the weak interaction, while CP is violated by the KobayashiMaskawa (KM) mechanism [5] with three generations of quarks. A complex phase in the CabibboKobayashiMaskawa (CKM) matrix provides the source of CP violation, which nicely describes all terrestrially observed CPviolating phenomena, that is, CP violation in the  and meson (even the meson) systems. (3) gauge symmetry is expected to be restored at high temperature above . Therefore, as the universe cools down to a temperature of around , the universe undergoes a phase transition (the EWPT) from symmetric phase of to the broken phase. If the EWPT is first order, the phase transition proceeds through bubble nucleation of the broken phase, where expansion of the bubbles fills up the entire universe. Thus, temporal departure from equilibrium is achieved near the surface of the expanding bubble.
Unfortunately, the measured parameters of the SM appear to be insufficient to bring about EWBG. The SM fails to explain the BAU due to two reasons. The first reason is that the KM mechanism with three quark generations cannot offer large enough CP violation (CPV) to produce the observed baryontoentropy ratio during the EWPT. The second reason is that the EWPT is not first order for a Higgs boson with GeV, required already by direct search at the LEP [6] and now indicated to be around 125 GeV at the LHC [7, 8]. Therefore, physics beyond the SM is needed for EWBG, and various extensions of the SM have been investigated from this point of view. In particular, there are extensive studies (for a recent review on EWBG, see [9]; and references therein) for the two Higgs doublet model and supersymmetric extensions of the SM, such as the MSSM and the NMSSM. It should be noted, however, that MSSM itself is under stress from the LHC, and its case for EWBG is only marginal [9]. One of the biggest means of attraction to have EWBG is that the implied new physics should be accessible at the LHC, at least partially.
In this contribution, we consider a fourgeneration (4G) extension of the SM and discuss a possibility to revive EWBG (beside a possible revival of EWBG, the 4G has another interesting implication on baryogenesis, if it is longlived; see [10]) fully within the SM framework, as 4G does not introduce anything that was not already contained in SM. We focus on the quark sector, which includes fourth generation quarks and . Compared to the threegeneration case, the 4G quarks bring three additional mixing angles and two additional complex phases in the CKM matrix, thus providing new sources of CP violation. One can argue intuitively for a possible effect of new CP violation on BAU by studying basisindependent invariants constructed from the quark mass matrices (or the Yukawa coupling matrices), which are extensions of the Jarlskog determinant in the SM. One of us [11] pointed out that such an invariant quantity can be highly enhanced compared to the threegeneration case, mainly due to the large masses (or the large Yukawa couplings) of and (see [12, 13] for an earlier discussion on 4Genhanced CP violation for BAU). As for the issue of the EWPT, a oneloop analysis shows that the 4G quarks do not play a positive role towards a firstorder phase transition [14]. However, given that bounds on the 4G quark masses from direct search at the LHC have entered 600 GeV level [15, 16], which is beyond the treelevel perturbative unitarity bound (UB) of 500–550 GeV [17], we have to reconsider the problem of EWPT beyond perturbation theory. In this regard, the nature of the EWPT with 4G quarks is still quite an open problem (for earlier works which address the issue of the EWPT within the fourgeneration framework (but not within the SM framework), see [14, 18] (supersymmetric model with the 4G fermions) and [19] (dynamical electroweak symmetry breaking model due to strong fourfermion interactions among the 4G fermions)).
The recent observation of a Higgslike object with mass around 125 GeV poses a special impasse situation, since a naive application of heavy and quarks in the loop would enhance the gluongluon fusion production of the Higgs boson by about an order of magnitude, which is not supported by data [7, 8], where is the or boson. Furthermore, quadratic corrections to the Higgs mass from heavy and quarks make the light Higgs mass rather difficult to sustain. With the deep conflict between a light Higgs and having 4G quarks beyond UB, it may seem cavalier to relegate this again to nonperturbative treatments. However, the aim of this work is very modest, which is just to show the nontrivial nature of 4G towards EWBG. Since the source of CPV arises from offdiagonal couplings, the Higgs boson does not directly enter EWBG computation. We will discuss towards the end the possibility that the observed 125 GeV boson could be a dilaton, rather than a bona fide SM Higgs boson, or it may be a pseudoGoldstone Higgs boson.
This paper is organized as follows. In Section 2, we discuss the effect of CP violation from the fourth generation quark sector on BAU. Extending the EWBG mechanism in the case of the SM to the fourth generation case, we estimate the amount of the BAU produced during a firstorder EWPT. In Section 3, we summarize the EWPT in the SM briefly and discuss possible mechanisms to induce a firstorder phase transition within the fourgeneration framework. Finally, in Section 4, we offer some discussions and give our summary.
2. CP Violation
One of the reasons for the failure of EWBG based on SM is the insufficiency of CP violation from the KM phase. This situation can be naively understood as follows.
In the SM with three generations, a basisindependent invariant for CP violation is given by the wellknown Jarlskog determinant [20], where are the up and downtype quark mass matrices. In terms of quark masses and CKM matrix elements, one gets where is twice the area of any triangle defined by the unitarity condition of the CKM matrix, , with the experimentally determined value of . One can estimate a naive strength of CP violation during the EWPT by constructing a dimensionless quantity from and the critical temperature, GeV. This gives , which is too small to account for BAU in (1).
It is readily observed that the smallness of originates mainly from the powers of light quark masses, , with milder suppression from the CKM factor . Motivated by this observation and a possible hint of new physics in transition, it was suggested in [11] to introduce the 4G quarks and replace (3) by an analogous quantity involving second to fourth generation quarks (or equivalently, treating the first two generations as degenerate), where . In fact, is a leading term of a basisindependent set of invariants for CP violation in the fourgeneration case and is given by , up to an overall factor [20, 21]. Due to heaviness of and , can be highly enhanced compared to in (3). For GeV, for instance, the enhancement factor reaches ~10^{18} solely from the mass factors, thus, seemingly possible to overcome the smallness of .
In the following, after we briefly review EWBG in the SM case, we take one step further and examine the previous expectation of 4Genhanced CP violation for the EWBG scenario.
A concrete mechanism of EWBG within SM was proposed by Farrar and Shaposhnikov (FS) [22–25]. In the FS mechanism, a baryon asymmetry is produced through CP violating scattering of quarks at the surface of an expanding bubble, that is, the bubble wall generated during a firstorder EWPT. CP asymmetry in reflection of the quarks off the bubble wall is induced by thermal effects, that is, interactions of the quarks with the and chargedHiggs bosons in the cosmic plasma. FS included these effects employing a quasiparticle picture and treated the scattering problem in a quantum mechanical manner. Solving an effective Dirac equation for the quasiparticles, they found that CP violation from the KM phase is sufficient to explain the BAU under optimal conditions, contrary to the naive argument given previous.
The very attractive SM explanation for BAU by FS was, however, refuted by subsequent works by Gavela et al. [26–28]. These authors pointed out that the width of the quasiparticle (damping rate) was not included in the study of FS, and they found that inclusion of the width reduces the baryon asymmetry to a negligible amount. This result was also confirmed by Huet and Sather (HS) [29], who interpreted the damping as quantum decoherence phenomenon induced by plasma effects, leading to reduction of the CP asymmetry, in which quantum mechanical coherence plays an essential role. After the demonstration of these results, it was (re)accepted that CP violation from the KM phase is not sufficient to explain BAU. This conclusion is in accordance with the naive dimensional argument of given previous. We now estimate, by extending the work of HS, the baryon asymmetry generated by the FS mechanism in the fourgeneration case.
We assume the existence of a firstorder phase transition. The baryon asymmetry generated during the firstorder EWPT is given by [29] where is the FermiDirac distribution, is the difference between lefthanded and righthanded quasiparticle momenta for a given energy , and is the velocity of the expanding bubble wall. We neglect contribution by assuming . We take GeV in the previous formula. is a reflection asymmetry defined by where reflection coefficients and are matrices in flavor space; that is, is the reflection coefficient for , where and refer to quark flavors, and corresponds to the CPconjugate process. provides the CP asymmetry for the reflection rate of a lefthanded quasiparticle, incident from the symmetric phase with an energy , summed over all flavors. We further assume that the EWPT is strongly first order, so that the generated baryon asymmetry is not washed out by the sphaleron processes in the broke phase (see next section). We return to discuss the issue of order of phase transition in 4G context later.
is obtained by solving an effective Dirac equation for the quasiparticles in the presence of spacedependent quark mass terms. Assuming planar wall with zero thickness, the effective Dirac equation is given by where , , and each are fourcomponent spinor wavefunctions. In (7), is a thermal mass matrix for the left (right) handed quasiparticles, is the quasiparticle width, and we use the one calculated in QCD [30], , neglecting possible flavordependent corrections from the Yukawa interactions.
Following HS, we solve the effective Dirac equations analytically based on the Green’s function method, which gives perturbative expansions of the reflection coefficients in terms of the quark mass matrices . The leadingorder contribution to from the scattering of the type quarks is given by where is the dominant part in the thermal masses of quarks, coming from QCD. The 4G effects enter solely through the last factor in (8), which arises as one follows the scattering of an incoming type quark against the bubble wall. In the threegeneration case, this factor is nothing but the Jarlskog determinant, discussed previous, where is defined in (2) and (3). On the other hand, the fourgeneration counterpart is more complicated, but it can be simplified [21] by exploiting the hierarchical structure of the quark masses and the CKM matrix elements, with a mild assumption on new mixings, (). Then, the last factor in (8) is approximated as where . One notes that , where is defined in (4). Therefore, can be actually enhanced by large masses of and compared to the SM case, as anticipated in [11].
As discussed by HS, dimensionless perturbative expansion parameters in the Green’s function method are given by , which are of order unity or larger for the , , and quarks, given GeV during the EWPT. Hence, the perturbative expansion breaks down for these heavy quarks, and the previous result for could be reduced due to large (equation (8) is obtained by the expansion in the type quark mass matrix based on the Green’s function method. The type quark mass matrix in (8) originates from the thermal mass matrix for the type quasiparticles, that is, the Yukawa interaction with the plasma. Thus, the heaviness of only the quark matters to ) if the perturbation is not used. Thus, the previous result might overestimate the CP asymmetry from the type quarks. The type quark contribution, at leading order, is the same as (8) except for the difference of the overall sign, hence, leading to a complete cancelation at this level. The previous mentioned remark is, however, also applied for the type quark contribution, and a possible amount of reduction would be even larger as it contains the contributions from the two heavy quarks, and . We naively accept (8) as a dominant contribution to the reflection asymmetry , simply neglecting the type quark contribution (there is another type of major contribution to , called in HS, which arises when the finite quark masses in the broken phase are taken into account in the selfenergy of quarks. While gives larger contribution to the BAU than (8) in the threegeneration case, we confirmed that the contribution from (8) dominates in the fourgeneration case for experimentally allowed masses of 4G quarks).
Eventually, the baryon asymmetry generated during the EWPT is given by where GeV and GeV are adopted. includes new CKM parameter which can be measured via flavor observables related with transition. We note that measurements for the CP violating phase in mixing, the forwardbackward asymmetry for , and the rate are making rapid progress at the LHC. Theoretical predictions for these observables are not subject to hadronic uncertainties so much; hence, they are useful to constrain [31]. From the recent LHC data, of around with GeV seems to be at the border of the experimentally allowed region [32]. However, with rising (and ), there is a tendency that drops, but the high powers of in (11) should easily compensate for it.
With reasonable 4G parameters, therefore, the FS mechanism with 4G quarks seems to generate the correct order of magnitude of the baryontoentropy ratio and, hence, can in principle explain BAU. We note that the previous estimate of BAU relies on the perturbative treatments of the Yukawa couplings/masses of the quarks including and in a few steps, while the LHC bounds on the 4G quark masses suggest a nonperturbative nature of the corresponding Yukawa couplings. For instance, the Green’s function method invokes the perturbation in the quark mass matrices as we already discussed. Besides this point, the thermal properties for the quasiparticles are obtained via perturbative calculations; for example, the thermal mass matrices are evaluated at oneloop level. Therefore, our result would be semiquantitative at most. Nevertheless, given remarkable enhancement of the CP asymmetry due to the 4G quarks and the agreement with the observed BAU as shown in (11), our finding should deserve further investigation. We further remark that the CPviolating Jarlskoglike invariants of (2) and (10) are of purely algebraic nature. Thus, we suspect that a fully dynamical calculation should still reflect this fact.
3. Electroweak Phase Transition
Besides CP violation, the other essential issue for EWBG is the nature of the EWPT. EWBG requires firstorder EWPT, which proceeds through nucleation and growth of brokenphase bubbles. In addition, there is a stronger requirement [12, 13] on the EWPT as explained later.
In EWBG, the baryon asymmetry is generated at the EWPT utilizing the violating sphaleron transition. However, the sphaleron transition must decouple just after the phase transition, otherwise the generated baryon asymmetry would be washed out. In the broken phase, the sphaleron transition rate is proportional to the Boltzmann factor , where is the energy of a sphaleron configuration and is given by , where is the thermal average of the Higgs field, , and is the SU(2) gauge coupling. In order to ensure the decoupling of the sphaleron transition in the broken phase, should be large enough to suppress the previous rate, leading to the condition , where is given by . Therefore, the firstorder EWPT has to be strong enough to avoid a washout of the generated baryon asymmetry.
A basic tool to analyze the EWPT is the finite temperature effective potential (FTEP) ([33–35], and for a review on EWPT and FTEP, see [36] and references therein). In SM, the oneloop FTEP is given by where is the treelevel potential for the Higgs field, is the temperature independent oneloop contribution, and represents the finite temperature correction to the zerotemperature potential. in Landau gauge and scheme is given by the ColemanWeinberg potential where is the dependent squared mass for particle with the corresponding number of degrees of freedom. See Table 1 for the definitions, where we note that fermions contribute with opposite sign.

The oneloop finite temperature contribution, , is given by where and are defined by In the high temperature limit where , can be expanded in terms of (hightemperature expansion) as where , and , that is, and .
Using high temperature expansion, the oneloop FTEP can be written as where Here, with GeV are physical masses for particle , and , as well as . In (17), terms which do not have dependence are omitted. For sake of illustration, we also neglect contributions from and by assuming that is lighter than and , though this is phenomenologically not correct. One sees that only weak bosons contribute to the coefficient of the cubic term in (17); hence, is rather small in SM.
With this FTEP, one can examine the behavior of the EWPT analytically. For , the only minimum of the effective potential, (17), is . Hence, the electroweak symmetry is restored. As the electroweak symmetry is broken at , the phase transition must occur at a temperature that satisfies . Inspection of (17), one clearly sees that the phase transition is first order for , taking the form depicted in Figure 1, and is second order for . When , the critical temperature and are given by Then, the strength of the firstorder phase transition is given by One notes that a lighter Higgs boson is preferred to maintain a stronger firstorder phase transition.
At high temperature, a certain class of higherorder diagrams, the socalled ring diagrams (or daisy diagrams) [36], give significant contributions to the FTEP. Dominant contributions from the ringdiagrams can be resummed, and it amounts to shifting the masses for bosons in the oneloop contributions, given in (13) and (14), to thermal masses given by , where is the oneloop selfenergy of particle in the infrared limit. As for gauge bosons, only the longitudinal modes receive corrections to the masses when oneloop selfenergies are adopted for . Basically, this forbids the longitudinal modes of and to contribute to the cubic term in (17). As a consequence, the coefficient of the cubic term is reduced as leading to the reduction of the strength of the EWPT.
With these results, the sphaleron decoupling condition, , reads However, this condition conflicts with the mass bound from direct search at the LEP, GeV [6]. Furthermore, recent results from the LHC indicate a Higgslike particle at 125 GeV. So, the EWPT is not strongly first order in the SM, and the baryon asymmetry generated during EWPT cannot be retained in the broken phase.
For a heavier Higgs boson, , the approximations used in the previous analysis are no longer correct in the SM. In particular, higherorder diagrams beyond the ring diagrams also become nonnegligible at critical temperature, and a nonperturbative analysis is required. Lattice studies [37–40] suggest, however, that there is an endpoint of firstorder EWPT around GeV, above which the transition turns into a continuous crossover. Therefore, there is no EWPT for the experimentally preferred Higgs boson mass.
For successful EWBG, then, physics beyond the SM is also required. It is clear that the existence of the cubic term in the FTEP of (17) is essential for a firstorder phase transition, and the cubic term arises from term in the high temperature expansion for the bosonic loop function , given in (16), while there is no such term from fermionic contributions. So, if a new boson with strong coupling to the Higgs boson is introduced, their thermal loop can enhance the cubic term, and the EWPT can be strengthened. On the other hand, introducing a new fermion does not affect the cubic term and, hence, does not improve the strength of the EWPT at oneloop level.
Based on the oneloop result, therefore, the introduction of 4G fermions seems useless from the viewpoint of making a firstorder EWPT. However, given that bounds on the 4G quark masses from direct search at the LHC have reached beyond the 600 GeV level, that is, beyond the perturbative unitarity bound of 500–550 GeV, we have to reconsider the problem of the EWPT beyond perturbative level. Interestingly, several studies (for zero temperature case) suggest that strong Yukawa couplings of 4G quarks can induce new bound states of 4G quarks [41–43]. If such Yukawa bound states are bound tightly enough so that they do not dissolve around the critical temperature of the EWPT, bosonic bound states may contribute to the FTEP via loop effect and may induce the cubic term, leading to strongly firstorder phase transition. Beside this possibility, if the 4G quarks form a pair condensate, , due to strong Yukawa couplings, an effective description of the theory would be given by a three Higgs doublet model (1 elementary + 2 composite Higgs doublet) [41] (the EWPT in multicomposite Higgs doublet model with the 4G fermions was studied in [19], where the composite Higgs fields appear as bound states of the 4G fermions, formed by strong fourfermion interactions). Therefore, the potential for the Higgs field would be modified even at tree level, and dynamics of the EWPT could be drastically changed.
4. Discussion and Summary
Let us continue the discussion from the previous section. Bosonization is only one aspect of very heavy 4G quarks that could change the landscape for EWBG. After all, the bosonization described previous is due to strong Yukawa coupling. A special feature of the SM is that fermion, in fact all, masses reflect a dynamical coupling. But fermions are special in that there is no theory of these Yukawa couplings, and, neglecting neutrinos, they span a range of six orders of magnitude! If a fourth generation exists above the unitarity bound, the strong Yukawa coupling could induce condensation, which in principle could replace the usual condensation of the Higgs field as the electroweak symmetry breaking mechanism. A “bootstrap” dynamical symmetry breaking (DSB) equation was recently formulated [44] and studied [45], and it was found numerically that DSB can occur for Yukawa coupling . For such strong Yukawa coupling, our traditional notions for EWBG may have to be reconsidered.
The difficulty for the bootstrap DSB scenario is again the newly observed [7, 8] 125 GeV boson at the LHC. However, the observed state could be a dilaton of scale invariance violation, rather than the genuine SM Higgs boson. The couplings of the dilaton to vector bosons and fermions are suppressed by compared to the SM Higgs boson case, where is the dilaton decay constant, while and couplings of the dilaton are essentially free parameters depending on the details of scale invariance violation [46]. Therefore, if the observed signal arises mostly from the gluon fusion, the dilaton could mimic the SM Higgs boson. Discrimination is provided by the detection of the Higgs production through the vector boson fusion (VBF), or the bremsstrahlung off a vector boson (VH). In particular, important modes are the VBFproduced mode and the and modes in this regard. As VBF and VH production are subdominant compared with gluon fusion, these modes are not yet firmly established by the LHC experiments. It is interesting that the bootstrap DSB equation is scale invariant by construction, and at the present level of study, the scale is introduced heuristically as a physical condition for the bootstrap [45]; hence, a dilaton is in principle allowed. Whether the 125 GeV state is the SMlike Higgs or a dilaton with rather modified couplings can be checked by ATLAS and CMS.
Even if the 125 GeV object is verified as SMlike Higgs boson, the strong Yukawa coupling of 4G quarks may still be relevant. The lightness of the Higgs boson may be because it is a pseudoGoldstone boson from a TeV scale strongly coupled theory, which indeed the previous situation seems to qualify it as a candidate. PseudoGoldstone Baryogenesis (PGBG) has been advocated [47] as a possible mechanism, where strong coupling brings about parametric enhancement of effective dimensionsix interactions that loosen the relation between Higgs selfcoupling and the Higgs mass; it is that really appears in (20), and Higgs mass enters only through the standard relation of . Thus, whether one could have PGBG at work or not has to be tested by checking the Higgs boson selfcoupling, which likely can be done only at an Linear Collider with energy above 500 GeV, which will take several decades.
Of course, the formulation of the bootstrap DSB equation is not yet at the level to demonstrate a possible PGBG, and much more work needs to be done. The formulation of the bootstrap DSB equation itself may offer a different path towards the study of order of phase transition. The equation is a coupled set of two integral equations of loop momentum in the ladder approximation [45]. At finite temperature, these would become four equations, since the temporal integration would be replaced by a summation. One could check the temperature dependence of DSB, both in finding the critical when symmetry is restored, but also check what is “,” the critical Higgs field expectation value, and whether its strength allows a strongly firstorder transition. Of course, this is not yet done, but it may offer further insight that is along a different path than the usual approach of [36] discussed in the previous section.
To summarize, EWBG is an attractive scenario to address the BAU puzzle, especially because this scenario is based on particle physics models that can be tested at the LHC. Although the EWBG scenario fails within the minimal SM with three quark generations, introduction of the fourth generation may revive the scenario, offering hope to solve the problems in the SM case. CP violation coming from the CKM matrix would be highly enhanced compared to the SM, mainly through the large masses (or the large Yukawa couplings) of and quarks. Naive extension of the EWBG mechanism of SM to the 4G case shows that this CP violating effect can be large enough to explain BAU with reasonable 4G parameters. The issue of whether the EWPT becomes strongly first order with 4G quarks is still an open problem, especially since the bounds on 4G quark masses from direct search at the LHC have reached the 600 GeV level, which is beyond the perturbative unitarity bound of 500–550 GeV. A mechanism of the strongly firstorder phase transition may be accommodated by new bound states and/or condensation of 4G quarks, both induced by strong Yukawa couplings, which could modify the FTEP at loop/tree level. Higgs boson search at the LHC has uncovered a new boson with SM Higgs features. The study is still ongoing, and its nature is important to obtain better understanding for the EWPT. All in all, the possibility of providing both sufficient CP violation as well as perhaps a strongly firstorder phase transition (which we did not demonstrate), all rooted in large Yukawa couplings of fourth generation quarks, makes this a worthy pursuit.
Acknowledgments
The authors are grateful to Y. Kikukawa for collaboration on the FS mechanism in the fourgeneration case, presented in Section 2. M. Kohda is supported by the NTU Grant no. 10R40044 and the Laurel Program, and W.S. Hou by the Academic Summit Grant NSC 1002745M002002ASP of the National Science Council of Taiwan and various NTU grants under the Excellence Program of the Ministry of Education of Taiwan.
References
 J. Beringer, J. F. Arguin, R. M. Barnett et al., “Review of particle physics,” Physical Review D, vol. 86, Article ID 010001, 2012. View at: Publisher Site  Google Scholar
 A. D. Sakharov, “CP symmetry violation, Casymmetry and baryonic asymmetry of the universe,” Zhurnal Eksperimentalnoi i Teoreticheskoi Fiziki, Pisma, vol. 5, p. 32, 1967. View at: Google Scholar
 A. D. Sakharov, “CP symmetry violation, Casymmetry and baryonic asymmetry of the universe,” Journal of Experimental and Theoretical Physics Letters, vol. 5, p. 24, 1967. View at: Google Scholar
 V. A. Kuzmin, V. A. Rubakov, and M. E. Shaposhnikov, “On anomalous electroweak baryonnumber nonconservation in the early universe,” Physics Letters B, vol. 155, no. 12, pp. 36–42, 1985. View at: Google Scholar
 M. Kobayashi and T. Maskawa, “CPViolation in the renormalizable theory of weak interaction,” Progress of Theoretical Physics, vol. 49, no. 2, pp. 652–657, 1973. View at: Google Scholar
 R. Barate, R. Bruneliere, I. de Bonis et al., “Search for the standard model higgs boson at LEP,” Physics Letters B, vol. 565, pp. 61–75, 2003. View at: Google Scholar
 G. Aad, T. Abajyan, B. Abbott et al., “Observation of a new particle in the search for the Standard Model Higgs boson with the ATLAS detector at the LHC,” Physics Letters B, vol. 716, no. 1, pp. 1–29, 2012. View at: Publisher Site  Google Scholar
 S. Chatrchyan, V. Khachatryan, A. M. Sirunyan et al., “Observation of a new boson at a mass of 125 GeV with the CMS experiment at the LHC,” Physics Letters B, vol. 716, no. 1, pp. 30–61, 2012. View at: Publisher Site  Google Scholar
 D. E. Morrissey and M. J. RamseyMusolf, “Electroweak baryogenesis,” New Journal of Physics, vol. 14, Article ID 125003, 2012. View at: Publisher Site  Google Scholar
 H. Murayama, V. Rentala, J. Shu, and T. T. Yanagida, “Saving fourth generation and baryon number by living long,” Physics Letters B, vol. 705, no. 3, pp. 208–211, 2011. View at: Publisher Site  Google Scholar
 W. S. Hou, “Source of CP violation for baryon asymmetry of the universe,” Chinese Journal of Physics, vol. 47, p. 134, 2009. View at: Google Scholar
 M. E. Shaposhnikov, “Possible appearance of the baryon asymmetry of the universe in an electroweak theory,” Jounal of Experimental and Theoretical Physics Letters, vol. 44, no. 8, pp. 465–468, 1986. View at: Google Scholar
 M.E. Shaposhnikov, “Baryon asymmetry of the universe in standard electroweak theory,” Nuclear Physics B, vol. 287, pp. 757–775, 1987. View at: Publisher Site  Google Scholar
 R. Fok and G. D. Kribs, “Four generations, the electroweak phase transition, and supersymmetry,” Physical Review D, vol. 78, no. 7, Article ID 075023, 2008. View at: Publisher Site  Google Scholar
 S. Chatrchyan, V. Khachatryan, A. M. Sirunyan et al., “Search for heavy, toplike quarkpair production in the dilepton final state in pp collisions at sqrt(s) = 7 TeV,” Physics Letters B, vol. 716, pp. 103–121, 2012. View at: Google Scholar
 S. Chatrchyan, V. Khachatryan, A. M. Sirunyan et al., “Search for heavy bottomlike quarks in 4.9 fb^{−1} of pp collisions at $\sqrt{\text{s}}=7$ TeV,” Journal of High Energy Physics, vol. 1205, p. 123, 2012. View at: Publisher Site  Google Scholar
 M. S. Chanowitz, M. A. Furman, and I. Hinchliffe, “Weak interactions of ultra heavy fermions,” Physics Letters B, vol. 78, no. 23, pp. 285–289, 1978. View at: Google Scholar
 S. W. Ham, S. K. Oh, and D. Son, “Electroweak phase transition in the minimal supersymmetric standard model with four generations,” Physical Review D, vol. 71, Article ID 015001, 6 pages, 2005. View at: Publisher Site  Google Scholar
 Y. Kikukawa, M. Kohda, and J. Yasuda, “The strongly coupled fourth family and a firstorder electroweak phase transition. I—quark sector,” Progress of Theoretical Physics, vol. 122, no. 2, pp. 401–426, 2009. View at: Publisher Site  Google Scholar
 C. Jarlskog, “Flavor projection operators and applications to CP violation with any number of families,” Physical Review D, vol. 36, no. 7, pp. 2128–2136, 1987. View at: Publisher Site  Google Scholar
 W. S. Hou, Y. Y. Mao, and C. H. Shen, “Leading effect of CP violation with four generations,” Physical Review D, vol. 82, Article ID 036005, 10 pages, 2010. View at: Publisher Site  Google Scholar
 G. R. Farrar and M. E. Shaposhnikov, “Baryon asymmetry of the universe in the minimal standard model,” Physical Review Letters, vol. 70, no. 19, pp. 2833–2836, 1993. View at: Publisher Site  Google Scholar
 G. R. Farrar and M. E. Shaposhnikov, “Erratum ‘Baryon asymmetry of the universe in the minimal standard model’,” Physical Review Letters, vol. 71, p. 210, 1993. View at: Google Scholar
 G. R. Farrar and M. E. Shaposhnikov, “Baryon asymmetry of the universe in the standard electroweak theory,” Physical Review D, vol. 50, no. 2, pp. 774–818, 1994. View at: Publisher Site  Google Scholar
 G. R. Farrar and M. E. Shaposhnikov, “Note added to ‘Baryon asymmetry of the universe in the standard model’,” http://arxiv.org/abs/hepph/9406387. View at: Google Scholar
 M. B. Gavela, P. Hernandez, J. Orloff, and O. Pene, “Standard model Cpviolation and baryon asymmetry,” Modern Physics Letters A, vol. 9, no. 9, p. 795, 1994. View at: Publisher Site  Google Scholar
 M. B. Gavela, M. Lozano, J. Orloff, and O. Pène, “Standard model CPviolation and baryon asymmetry (I). Zero temperature,” Nuclear Physics B, vol. 430, no. 2, pp. 345–381, 1994. View at: Google Scholar
 M. B. Gavela, P. Hernandez, J. Orloff, O. Pène, and C. Quimbay, “Standard model CPviolation and baryon asymmetry (II). Finite temperature,” Nuclear Physics B, vol. 430, no. 2, pp. 382–426, 1994. View at: Google Scholar
 P. Huet and E. Sather, “Electroweak baryogenesis and standard model CP violation,” Physical Review D, vol. 51, no. 2, pp. 379–394, 1995. View at: Publisher Site  Google Scholar
 E. Braaten and R. D. Pisarski, “Calculation of the quark damping rate in hot QCD,” Physical Review D, vol. 46, no. 4, pp. 1829–1834, 1992. View at: Publisher Site  Google Scholar
 W. S. Hou, M. Kohda, and F. Xu, “Measuring the fourthgeneration b→s quadrangle at the LHC,” Physical Review D, vol. 84, no. 9, Article ID 094027, 7 pages, 2011. View at: Publisher Site  Google Scholar
 W. S. Hou, M. Kohda, and F. Xu, “Hints for a low ${B}_{s}\to {\mu}^{+}{\mu}^{}$ rate and the fourth generation,” Physical Review D, vol. 85, no. 9, Article ID 097502, 5 pages, 2012. View at: Publisher Site  Google Scholar
 L. Dolan and R. Jackiw, “Symmetry behavior at finite temperature,” Physical Review D, vol. 9, no. 12, pp. 3320–3341, 1974. View at: Publisher Site  Google Scholar
 S. Weinberg, “Gauge and global symmetries at high temperature,” Physical Review D, vol. 9, no. 12, pp. 3357–3378, 1974. View at: Publisher Site  Google Scholar
 G. W. Anderson and L. J. Hall, “Electroweak phase transition and baryogenesis,” Physical Review D, vol. 45, no. 8, pp. 2685–2698, 1992. View at: Publisher Site  Google Scholar
 M. Quiros, “Finite temperature fieldtheory and phase transitions,” http://arxiv.org/abs/hepph/9901312. View at: Google Scholar
 M. Gürtler, E. M. Ilgenfritz, and A. Schiller, “Where the electroweak phase transition ends,” Physical Review D, vol. 56, no. 7, pp. 3888–3895, 1997. View at: Google Scholar
 M. Laine and K. Rummukainen, “What's new with the electroweak phase transition?” Nuclear Physics B, vol. 73, no. 1–3, pp. 180–185, 1999. View at: Google Scholar
 F. Csikor, Z. Fodor, and J. Heitger, “End point of the hot electroweak phase transition,” Physical Review Letters, vol. 82, no. 1, pp. 21–24, 1999. View at: Google Scholar
 Y. Aoki, F. Csikor, Z. Fodor, and A. Ukawa, “The end point of the firstorder phase transition of the SU(2) gaugeHiggs model on a 4dimensional isotropic lattice,” Physical Review D, vol. 60, no. 1, Article ID 013001, pp. 1–8, 1999. View at: Google Scholar
 P. Q. Hung and C. Xiong, “Dynamical electroweak symmetry breaking with a heavy fourth generation,” Nuclear Physics B, vol. 848, no. 2, pp. 288–302, 2011. View at: Publisher Site  Google Scholar  Zentralblatt MATH
 K. Ishiwata and M. B. Wise, “Fourth generation bound states,” Physical Review D, vol. 83, no. 7, Article ID 074015, 8 pages, 2011. View at: Publisher Site  Google Scholar
 T. Enkhbat, W. S. Hou, and H. Yokoya, “Early LHC phenomenology of Yukawabound heavy $Q\overline{Q}$ mesons,” Physical Review D, vol. 84, no. 9, Article ID 094013, 14 pages, 2011. View at: Publisher Site  Google Scholar
 W. S. Hou, “Some unfinished thoughts on strong yukawa couplings,” Chinese Journal of Physics, vol. 50, p. 375, 2012. View at: Google Scholar
 Y. Mimura, W. S. Hou, and H. Kohyama, “Bootstrap dynamical symmetry breaking with new heavy chiral quarks,” http://arxiv.org/abs/1206.6063. View at: Google Scholar
 D. Elander and M. Piai, “The decay constant of the holographic technidilaton and the 125 GeV boson,” Nuclear Physics B, vol. 867, no. 3, pp. 779–809, 2013. View at: Google Scholar
 B. Grinstein and M. Trott, “Electroweak baryogenesis with a pseudoGoldstone Higgs boson,” Physical Review D, vol. 78, no. 7, Article ID 075022, 28 pages, 2008. View at: Publisher Site  Google Scholar
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Copyright © 2013 WeiShu Hou and Masaya Kohda. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.