Sphalerons and the Electroweak Phase Transition in Models with Higher Scalar Representations

# Sphalerons and the Electroweak Phase Transition in Models with Higher Scalar Representations

Amine Ahriche Department of Physics, University of Jijel, PB 98 Ouled Aissa, DZ-18000 Jijel, AlgeriaFakultät für Physik, Universität Bielefeld, 33501 Bielefeld, GermanyThe Abdus Salam International Centre for Theoretical Physics, Strada Costiera 11, I-34014, Trieste, ItalySISSA, Via Bonomea 265, 34136, Trieste, ItalyDepartment of Physics, UAE University, P.O. Box 17551, Al-Ain, United Arab Emirates    Talal Ahmed Chowdhury Department of Physics, University of Jijel, PB 98 Ouled Aissa, DZ-18000 Jijel, AlgeriaFakultät für Physik, Universität Bielefeld, 33501 Bielefeld, GermanyThe Abdus Salam International Centre for Theoretical Physics, Strada Costiera 11, I-34014, Trieste, ItalySISSA, Via Bonomea 265, 34136, Trieste, ItalyDepartment of Physics, UAE University, P.O. Box 17551, Al-Ain, United Arab Emirates    and Salah Nasri Department of Physics, University of Jijel, PB 98 Ouled Aissa, DZ-18000 Jijel, AlgeriaFakultät für Physik, Universität Bielefeld, 33501 Bielefeld, GermanyThe Abdus Salam International Centre for Theoretical Physics, Strada Costiera 11, I-34014, Trieste, ItalySISSA, Via Bonomea 265, 34136, Trieste, ItalyDepartment of Physics, UAE University, P.O. Box 17551, Al-Ain, United Arab Emirates
###### Abstract

In this work we investigate the sphaleron solution in a gauge theory, which also encompasses the Standard Model, with higher scalar representation(s) (). We show that the field profiles describing the sphaleron in higher scalar multiplet, have similar trends like the doublet case with respect to the radial distance. We compute the sphaleron energy and find that it scales linearly with the vacuum expectation value of the scalar field and its slope depends on the representation. We also investigate the effect of gauge field and find that it is small for the physical value of the mixing angle, and resembles the case for the doublet. For higher representations, we show that the criterion for strong first order phase transition, , is relaxed with respect to the doublet case, i.e. .

###### Keywords:
sphalerons, scalar multiplets.

## 1 Introduction

In the Standard Model (SM), the anomalous baryonic and leptonic currents lead to fermion number non-conservation due to the instanton induced transitions between topologically distinct vacua of gauge fields 'tHooft:1976up (); 'tHooft:1976fv () and at zero temperature, the rate is of the order, , , which is irrelevant for any physical phenomena. However, there exists a static unstable solution of the field equations, known as sphaleron Dashen:1974ck (); Manton:1983nd (); Klinkhamer:1984di (); Soni:1980ps (), that represents the top of the energy barrier between two distinct vacua and at finite temperature, because of thermal fluctuations of fields, fermion number violating vacuum to vacuum transitions can occur which are only suppressed by a Boltzmann factor, containing the height of the barrier at the given temperature, i.e. the energy of the sphaleron Kuzmin:1985mm (). Such baryon number violation induced by the sphaleron is one of the essential ingredients of Electroweak Baryogenesis Shaposhnikov:1987tw (); Shaposhnikov:1987pf (); Arnold:1987mh (); Khlebnikov:1988sr (); Dine:1989kt (); Dine:1991ck () and therefore it has been extensively studied not only in the SM Akiba:1988ay (); Akiba:1989xu (); Yaffe:1989ms (); Arnold:1987zg (); Carson:1990jm (); Klinkhamer:1990fi (); Kleihaus:1991ks (); Kunz:1992uh (); Brihaye:1992jk (); Braibant:1993is (); Brihaye:1993ud () and but also in extended SM variants such as, SM with a singlet Choi:1994mf (); Ahriche:2007jp (), two Higgs doublet model Kastening:1991nw (), Minimal Supersymmetric Standard Model Moreno:1996zm (), the next-to-Minimal Supersymmetric Standard Model Funakubo:2005bu () and 5-dimensional model Ahriche:2009yy ().

As many SM extensions involve non-minimal scalar sectors, it is instructive to determine the behavior of the sphaleron for general scalar representations. Although, apart from some exceptions like Georgi-Machacek Georgi:1985nv () and isospin-3 models Kanemura:2013mc (), large Higgs multiplets other than the doublet are stringently constrained by electroweak precision observables. In addition, the presence of scalar multiplets with isospin brings down the Landau pole of the gauge coupling to about TeV AbdusSalam:2013eya (). Moreover as shown in Hally:2012pu (); Earl:2013jsa (), by saturating unitarity bound on zeroth order partial wave amplitude for the scattering of scalar pair annihilations into electroweak gauge bosons, one can set complex multiplet to have isospin and real multiplet to have . Therefore it can be seen that large scalar representations of SM gauge group are generally disfavored.

Still, motivated by the dark matter content and baryon asymmetry of the universe, one can assume a hidden or dark sector with its own gauge interactions. If the interaction between SM and hidden sector is feeble in nature, they may not equilibrate in the whole course of the universe. Therefore, the hidden sector can be fairly unconstrained apart from its total degrees of freedom such that the sector doesn’t change the total energy density of the universe in such way that the universe had a modified expansion rate in earlier times, specially at the BBN and CMB era. With this possibility in mind, we can consider the hidden sector to have SM-like gauge structure that contains scalar multiplets larger than doublet and also has its own spontaneous symmetry breaking scale (the possibility of non-abelian gauge structure in dark sector and non-SM sphaleron in symmetric phase for such models are also addressed in Blennow:2010qp (); Barr:2013tea ()). For this reason, it is interesting to ask what could be the nature of the sphaleron in such SM-like gauge group with general scalar multiplets. Furthermore, as sphaleron is linked with nontrivial vacuum structure of non-abelian gauge theory, it is relevant to see the effect of large scalar multiplets in hot gauge theories.

This paper is organized as follows. In section 2 we discuss the spherically symmetric ansatz for larger scalar multiplets and consequently calculated the energy functional and variational equations for scalar multiplet , give different numerical results. In section 3 we investigate the effect of field on sphaleron energy and study the sphaleron energy dependence on the scalar vev. Section 4 is devoted to the conditions of the sphaleron decoupling during the electroweak phase transition, and in section 5 we conclude. In Appendix A, we have presented the asymptotic solutions and their dependence on the representation .

## 2 Sphalerons in General Scalar Representation

### 2.1 Spherically symmetric Ansatz

The standard way to find sphaleron solution in the Yang-Mills-Higgs theory is to construct non-contractible loops in field space Klinkhamer:1984di (). As the sphaleron is a saddle point solution of the configuration space, it is really hard to find them by solving the full set of equations of motion. Instead one starts from an ansatz depending on a parameter that characterizes the non-contractible loop in the configuration space and corresponds to the vacuum for and while corresponds the highest energy configuration, in other words, the sphaleron.

Consider the scalar multiplet , charged under group, is in representation and has charge . Here and can be applicable for both standard model gauge group or SM-like gauge group of the hidden sector. The generators in this representation are denoted as such that, where is the Dynkin index for the representation. As our focus is on the SM, we define the charge operator, and require the neutral component () of the multiplet to have the vacuum expectation value (vev).

The gauge-scalar sector of the Lagrangian is

 L=−14FaμνFaμν−14fμνfμν+(DμQ)†DμQ−V(Q), (1)

with scalar potential

 V(Q)=−μ2QQ†Q+λ1(Q†Q)2+λ2(Q†JaQ)2. (2)

It was shown in Ahriche:2007jp () that the kinetic term of the scalar field makes larger contribution to the sphaleron energy than the potential term. Therefore, for simplicity, we have considered CP-invariant scalar potential involving single scalar representation to determine the sphaleron solution. It is straightforward to generalize the calculation for the potential with multiple scalar fields111In fact, in the SM, one needs large couplings between Higgs and extra scalars to trigger a strong first order phase transition..

Also for convenience we elaborate,

 Faμν =∂μAaν−∂νAaμ+gϵabcAbμAcν, fμν =∂μaν−∂νaμ, DμQ =∂μQ−igAaμJaQ−ig′aμXQ, (3)

where, and are the and gauge couplings. The mixing angle is .

The scalar sector plays an essential role in constructing sphaleron and the symmetry features of the ansatz partly depends on the representation and charge assignment of the scalar that acquires a vev. The simplest possibility is to consider a spherically symmetric ansatz because spherical symmetry enables one to calculate the solution and the energy of the sphaleron without resorting into full partial differential equations. Therefore one may ask, which scalar representation immediately allows the spherical symmetric ansatz.

As pointed out in Yaffe:1989ms (), spherically symmetric configurations are those for which an rotation of spatial directions are compensated by the combination of gauge and global transformation. The existence of this global symmetry is manifest for the Higgs doublet as the potential for the doublet has global symmetry which is broken by the scalar vev to symmetry that leads to the mass degeneracy of three gauge bosons of . One can immediately see that this degeneracy will be lifted when the is turned on. Following the same reasoning, one can find other scalar multiplets that will lead to mass degeneracy of ’s in gauge theory after the symmetry is broken.

In the case of many scalar representations with and charge , the corresponding vev’s are , where the non-zero neutral component quantum numbers are . Now from the scalar kinetic term,

 L ⊃12g2∑i⟨Q(i)†⟩J(i)aJ(i)b⟨Q(i)⟩AaμAμb =12g2∑iv2i(J(i)(J(i)+1)−X(i)2)A+μAμ−+12g2∑iv2iX(i)2A3μAμ3. (4)

where . So the condition for having equal coupling of three gauge fields to the neutral component leads to the tree-level condition

 ρ=∑iv2i(J(i)(J(i)+1)−X(i)2)2∑iv2iX(i)2=1. (5)

In the case of one scalar multiplet, this can be reduced to . The multiplets satisfying the above condition are . Intuitively, one can consider that the scalar multiplet enables the three gauge fields to scale uniformly like a sphere in a three dimensional space.

### 2.2 The Energy Functional and Variational Equations

In the following we will address the energy functional and the variational equations of the sphaleron. The classical finite energy configuration are considered in a gauge where the time component of the gauge fields are set to zero. Therefore the classical energy functional over the configuration is

 E(Aai,ai,Q)=∫d3x[14FaijFaij+14fijfij+(DiQ)†(DiQ)+V(Q)]. (6)

The non-contractible loop (NCL) in configuration space is defined as map into using the following matrix Klinkhamer:1990fi (),

 U∞(μ,θ,ϕ) =(cos2μ+sin2μcosθ)I2+isin2μ(1−cosθ)τ3 +2isinμsinθ(sinϕτ1+cosϕτ2), (7)

where is the parameter of the NCL and , are the coordinates of the sphere at infinity. Also, are the generators in the fundamental representation. We also define the following 1-form

 i(U∞−1)dU∞=∑aFaτa, (8)

which gives

 F1 =−[2sin2μcos(μ−ϕ)−sin2μcosθsin(μ−ϕ)]dθ −[sin2μcos(μ−ϕ)sinθ+sin2μsin2θsin(μ−ϕ)]dϕ, F2 =−[2sin2μsin(μ−ϕ)+sin2μcosθcos(μ−ϕ)]dθ +[sin2μsin2θcos(μ−ϕ)−sin2μsinθsin(μ−ϕ)]dϕ, F3 =−sin2μsinθdθ+2sin2θsin2μdϕ. (9)

As shown in Klinkhamer:1990fi (), the NCL starts and ends at the vacuum and consists of three phases such that in first phase it excites the scalar configuration, in the second phase it builds up and destroys the gauge configuration and in the third phase it destroys the scalar configuration.

The field configurations in the first and third phases, and are

and

 Q=v(sin2μ+h(ξ)cos2μ)√2(0..1..0)T, (11)

with  is radial dimensionless coordinate and  is the mass parameter used to scale , which we choose in what follows as . In the second phase , the field configurations are

and

 Q=vh(ξ)√2(0..1..0)T. (13)

Here, , , and are the radial profile functions. From Eq.(12), one can see that in the spherical coordinate system, for the chosen ansatz, the gauge fixing has led to, . Moreover, similar to Eq.(12), the gauge fields acting on the scalar field can be written as

Finally the energy over the NCL for the first and third phases is,

 E(h,μ)=4πΩg∫∞0dξ[cos2μv2Ω212ξ2h′2+ξ2V(h,μ)g2Ω2], (15)

and for second phase,

 E(μ,f,f3,f0,h) =4πΩg∫∞0dξ[sin2μ(83f′2+43f′32)+8ξ2sin4μ{23f23(1−f)2 +13{f(2−f)−f3}2}+43(gg′)2{sin2μf′02+2ξ2sin4μ(1−f0)2} +v2Ω2{12ξ2h′2+43sin2μh2{(J(J+1)−J23)(1−f)2+J23(f0−f3)2}} +ξ2g2Ω4V(h)]. (16)

From Eq.(16), the maximal energy is attained at which corresponds to the sphaleron configuration.

If there are multiple representations with non-zero neutral components ,
, the energy of the sphaleron can be parameterized as

 Esph =E(μ=π2)=4πΩg∫∞0dξ[[83f′2+43f′32+83ξ2{2f23(1−f)2 +(f(2−f)−f3)2}+43(gg′)2{f′02+2ξ2(1−f0)2}+∑i{12v2iΩ2ξ2h′i2 +43h2i[2αi(1−f)2+βi(f0−f3)2]}+ξ2V(vihi)g2Ω4], (17)

where the parameters

 αi=(J(i)(J(i)+1)−J(i)23)v2i2Ω2, βi=J(i)23v2iΩ2, (18)

refer to the scalar field couplings to the charged and neutral gauge fields respectively.

The energy functional, Eq.(17) will be minimized by the solutions of the following variational equations

 f′′+2ξ2(1−f)[f(f−2)+f3(1+f3)]+∑iαih2i(1−f)=0, f′′3−2ξ2[3f3+f(f−2)(1+2f3)]+∑iβih2i(f0−f3)=0, f′′0+2ξ2(1−f0)−g′2g2∑iβih2i(f0−f3)=0, h′′i+2ξh′i−8Ω23v2iξ2hi[2αi(1−f)2+βi(f0−f3)2]−1g2viΩ2∂∂ϕiV(ϕ)∣∣∣ϕk=vkhk=0, (19)

with the boundary conditions for Eq.(19) are given by: , and . For , we have, and for representations satisfying Eq.(5), . The behavior of the field profiles Eq.(19) at the limits and  are shown in Appendix A. According to the last term in both first and second lines in Eq.(19), it seems that the couplings of the scalar to gauge components, i.e. Eq.(18) will play the most important role in the profile’s shape as well as in the sphaleron energy. The equality between the parameters and leads to the case Eq.(5) and any difference between and will characterize a splitting between the functions and , and therefore a departure from the spherical ansatz that was defined in Klinkhamer:1984di ().

### 2.3 Numerical Results

Here we are interested in investigating the properties of the field profiles for different scalar representations and vevs. First we have studied the field profiles for only with scalar representation where is taken to be zero and consequently . The scalar representations are taken as , , , , , , , and two scalar vevs: GeV and GeV. Here we are focusing on the sphaleron solution in a generic case; therefore, we have chosen representative values of the vev which also contain the SM case, GeV within the range. Moreover, for each representation, the quartic coupling is set to be 0.12 and the mass parameter is determined by coupling and the scalar vev. For this parameter set, the mass of the scalar field remains smaller than so there is no appearance of bisphalerons in our case. The field profiles are given in Figure 1.

According to Figure 1, one can make the following remarks:

• Comparing the cases of small vev, GeV and large vev, GeV, it can be seen that all field profiles tend quickly to the unity as the vev gets larger. This could explain the dependence of sphaleron energy Eq.(17) on the scalar vev.

• When the scalar representation is large (large so that large ), the profile for charged gauge field (i.e., ) tends to faster with , in contrast with the scalar field profile, .

• For the neutral gauge field profile , it is identical to for the representation () because it satisfies  (or ) condition.

• For the same value of the vev and the isospin , the field profile tends to 1 faster for larger values of , i.e. larger values of .

• The scalar field profiles seem to be not sensitive to the values of .

Therefore, it is seen that the gauge field profiles tend to unity faster in contrast to the scalar field profiles with radial coordinate for large couplings of the scalar to charged gauge boson, and neutral gauge boson, . In the next section, we will see the impact of this feature on the sphaleron energy.

## 3 The Effect of U(1)x Field and the Sphaleron Energy

In the presence of a non-zero gauge coupling or non-zero Weinberg angle , the gauge field will be excited and the spherical symmetry will be reduced to axial symmetry. In Brihaye:1992jk (), it was shown for the SM with one Higgs doublet that when the mixing angle is increased, the energy of the sphaleron decreases and it changes the shape from a sphere at to a very elongated spheroid at large mixing angle. However, for the physical value of the mixing angle, the sphaleron differs only little from the spherical sphaleron. On the other hand, for multiplets not satisfying Eq.(5), the shape of the corresponding sphaleron will be spheriodal instead of spherically symmetric in the case. In such cases, the large value of the mixing angle may be significant for the energy and shape of the sphaleron for large multiplet future (). In the following, we have adopted the small mixing angle scenario so that sphalerons are not so different than the case; and we will work at first order of small value.

In Figure 2, we have presented the field profile for different values of vev ( GeV) and different representations ().

In the case of a sphaleron, we have presented only the field profile since the other profiles (, and ) are very close to the case of vanishing Weinberg angle shown in the previous section. In Figure 2, one can notice that the field profile is just a deviation from unity similar to the singlet scalar profile in models with singlets Ahriche:2007jp () and it gets closer to unity as the values becomes smaller and smaller. Indeed, it is exactly one for the representations and which means that in those cases the sphaleron energy is not affected by the existence of gauge field.

When we have , even when one starts with , the following current will induce ,

 ji=i2g′[Q†DiQ−(DiQ)†Q], (20)

In the leading order approximation of , we can neglect the contribution in the covariant derivative. Therefore the non-zero component of the current in the chosen ansatz is Klinkhamer:1984di ()

 jϕ=g′sinθr∑iv2iJ(i)3h2i(1−f). (21)

Because of induced field , there will be a dipole contribution to the energy,

 Edipole =∫d3xaiji =−16π3gΩ∑iv2iJ(i)3∫∞0dξ(1−f0)(1−f)h2i, (22)

and the sphaleron energy will be

 Esph|θW≠0=Esph|θW=0+Edipole. (23)

In the current Eq.(21) the contribution of the gauge field is generally neglected in the literature and when we consider it, the current and the dipole energy become

 jϕ =g′sinθr∑iv2iJ(i)3h2i(f0−f3), E′dipole =−16π3gΩ∑iv2iJ(i)3∫∞0dξ(1−f0)(f0−f3)h2i, (24)

Therefore the dipole contribution Eq.(22) is expected to be almost equal to the difference between Eq.(17) and the same quantity with , i.e., . In order to probe this, we estimate the difference between the sphaleron energy in the non-zero and zero mixing cases in three different ways: (A) with is given in Eq.(17); (B) with field neglected as given in Eq.(22); and (C) as shown in Eq.(24). These three quantities are presented in function of the scalar vev in Figure 3.

Figure 3 shows the relative difference between the sphaleron energy with the mixing angle and and also the (negative) dipole energy of the sphaleron. It turns out that for any scalar representation, the relative difference between the sphaleron energy with and is always less than and remains constant for different values of scalar vev. However, when considering the gauge field effect on the dipole energy Eq.(24), it becomes closer to the exact difference.

Now we present the sphaleron energy Eq.(17) as a function of the scalar vev for different scalar representations as shown in Figure 4.

In Figure 4 we can see that the sphaleron energy depends on the scalar vev with a slope that depends on scalar isospin and hypercharge (or ). This allows us the write the scaling law as

 Esph(v,J,X)=Z(J,X)v, (25)

where the function represents the slope in Figure 4.

## 4 Sphaleron Decoupling Condition

Before the electroweak phase transition , the classical background scalar field, , is zero and the Universe is in the symmetric phase. In this phase, the sphaleron processes 222The term ”sphaleron processes” is used in the literature to refer to the baryon number violating processes which also have the CP violating feature. are in full thermal equilibrium and are given as Arnold:1996dy (); Bodeker:1998hm (); Arnold:1998cy (); Moore:2000mx ()

 Γsym∼α5wT4ln(1/αw), (26)

with is the weak coupling. Therefore any generated baryon asymmetry due to the sphaleron processes will be erased by the inverse process. Once the temperature drops below the critical one , bubbles of true vacuum () start to nucleate where the rate is suppressed as .

The sphaleron decoupling condition indicates that the rate of baryon number violation must be much smaller than the the Hubble parameter Shaposhnikov:1987tw (); Shaposhnikov:1987pf (); Bochkarev:1987wf () and therefore, the condition on the sphaleron rate is Arnold:1987mh (); Akiba:1989xu (); Funakubo:2009eg ()

 −1BdBdt≃13Nf128π2ω−α3wκNtrNrote−Esph/T

where is the baryon number density, the factors and come from the zero mode normalization, is the eigenvalue of the negative mode Carson:1989rf (). The factor is the functional determinant associated with fluctuations around the sphaleron Dine:1991ck (). It has been estimated to be in the range:  Carson:1990jm (); kapan (). The Hubble parameter is given as

 H(T)≃1.66√g∗(T)T2/Mpl, (28)

where and are the Planck mass and the effective number of degrees of freedom that are in thermal equilibrium.

It was shown in Braibant:1993is () for the doublet case that the sphaleron energy at a given temperature can be well approximated by the following relation

 Esph(v(T),T)v(T)=Esph(v0)v0, (29)

where is the vev of the scalar field at temperature and is its zero temperature value. Eq.(29) shows that a straightforward estimation of the sphaleron energy at finite temperature is possible by determining its energy at zero temperature. This means that the scaling law Eq.(25) is valid also at finite temperature case, where the function is temperature-independent. Because of similar linear scaling shown by higher scalar representations in Figure 4, we can use the scaling law Eq.(25) for other representations.

Hence, for general scalar representation, the decoupling of baryon number violation Eq.(27) implies the following relation Funakubo:2009eg ()

 v(Tc)Tc>1Z(J,X)[42.97+ln(κNtrNrot)+lnω−mW−12lng∗106.75−2lnTc100 {\normalsize{GeV }}]. (30)

Most of the parameters in the r.h.s of Eq.(30) are logarithmically model-dependent and therefore one can safely use the SM values. In the case of SM, we have Arnold:1987mh () and for , Carson:1989rf (); Carson:1990jm (); Akiba:1989xu (). It can be noted that the contributions of model dependent quantities in are smaller than , for example, in the SM Funakubo:2009eg () zero mode contribution is around and the contributions from the negative mode, relativistic degrees of freedom and critical temperature are about . For this reason we can consider the dominant contribution is coming from . In conjunction, using (or ), and GeV, we have from Eq.(30),

 v(Tc)Tc>ηJ,X, (31)

where is given for each scalar representation in Table-1.

It is clear that as the representation becomes larger, the strong first order phase transition criterion gets relaxed. Generally, the case of is the commonly used criterion in the literature. In a general case of a multi-scalars model with representations (), the criterion Eq.(31) can be generalized as

 Θ(Tc)Tc>1, (32)

with

 Θ(Tc)2=∑ivi(Tc)2η2J(i),X(i), (33)

with is the temperature dependent scalar vev of the multiplet . In order to check the criterion Eq.(33), we consider the case of a model with two scalar representations and estimate the ratio for different values of , , , , and while keep the W gauge boson mass constant. The ratio versus the ratio is shown in Figure 5.

From Figure 5, it is clear that the sphaleron energy scales like for different representations and vevs within the error less than 5.7 %; and if the values of the two vevs are comparable, this error is reduced to 2.7 %. Therefore, one can safely use Eq.(33) as a criterion for a strong first order phase transition in any model with multiscalars.

## 5 Conclusion

We have constructed the energy functional and relevant variational equations of the sphaleron for general scalar representation charged under gauge group and shown that the sphaleron energy increases with the size of the multiplet. Furthermore, it has been shown that at a fixed value of the vev, the sphaleron energy is large for larger representation and for each representation, it linearly scales with the vev. As the energy of the sphaleron increases with the size of the scalar representation, the criterion for the strong first order phase transition is relaxed for larger representation. We have presented a representation dependent criterion for strong phase transition which is relevant for the electroweak baryogenesis.

We have also found that the dipole approximation (with or without considering in the current, ) does not correspond exactly the energy difference and that is less than 2% for any scalar representation. In this case the field profile is just a deviation from unity and therefore just playing a relaxing role similar to singlet seen in Ahriche:2007jp ().

However, as we have seen in Figure 3 that the dipole contribution to the sphaleron energy is negative, its coupling with the external magnetic field produced in the bubbles of first order phase transition through the dipole moment would lower the sphaleron energy and thus strengthen the sphaleron transition inside the bubble and wash out the baryon asymmetry more efficiently as pointed out in DeSimone:2011ek (). A more careful analysis on this aspect for the sphaleron with higher scalar representation will be carried out in future ().

We have presented in Eq.(33) a general criterion for the strong first order phase transition in a model with multiple scalars of different representations and we have shown that this approximate criterion is valid with an error less than 5%.

## Acknowledgements

We are grateful to Goran Senjanović, Eibun Senaha, Andrea De Simone, Dietrich Bödeker and Xiaoyong Chu for the critical reading of the manuscript and helpful comments. T.A.C. would also like to thank Basudeb Dasgupta, Luca Di Luzio and Marco Nardecchia for discussion. A.A. is supported by the Algerian Ministry of Higher Education and Scientific Research under the CNEPRU Project No. D01720130042.

## Appendix A Asymptotic solutions

To capture the dependence of solutions on , in this section we have included the analytical estimates of solutions for the asymptotic region and . For the energy functional Eq.(17) to be finite, the profile functions should be , , and . Therefore, at , the equations Eq.(19) are reduced into

 ξ2f′′ −4f+2f3+αξ2h2=0, (34) ξ2f′′3 −6f3+4f+βξ2h2=0, (35) f′′0 +2(1−f0)−(g′g)2βξ2h2=0, (36) ξ2h′′ +2ξh′−8m3h=0, (37)

where

 m=Ω2v2(2α+β). (38)

The solution of Eq.(37) which leads to finite energy of the sphaleron is

 h(ξ)∼Aξ−12(1−p), (39)

with

 p=√1+323m. (40)

Now at , , so using this approximation, from Eq.(34) we have,

 f(ξ)∼Bξ2−4Aαξ12(3+p)(p2−1)(p2+5). (41)

On the other hand, we have considered as a perturbation in Eq.(35). Therefore, we have

 f3(ξ)∼Cξ3+Bξ2−Kξ12(3+p). (42)

Here, is defined as follows

 K=3A{3α(3p−8m+3)+8mβ(4m−9)}4m(4m−9)(8m+3p−15). (43)

Finally from Eq.(36), we have

 f0(ξ)∼1+Dξ2+3Aβg′2ξ12(3+p)g2(3p−8m+3), (44)

and , , and are integration constants.

On the other hand, for asymptotic region, , all the profile functions must approach unity to have finite energy of the sphaleron. So we consider the functions to be the small perturbation to unity as follows. Taking, , , and and keeping only the linear terms of the variation, we have

 δf′′−αδf =0, δf′′3+β(δf0−δf3) =0, δf′′0−g′2g2β(δf0−δf3) =0, ξ2δh′′−2ξδh−3λv2g2Ω2ξ2δh =0. (45)

The asymptotic solutions at are,

 f(ξ) ∼1+Ee−√αξ, f3(ξ) ∼1+Fe−√βξ, f0(ξ) ∼1+Ge−√βξ, h(ξ) ∼1+He−√3λvgΩξξ, (46)

where , , and are again integration constants. The constants from to depend on and couplings and they are determined by matching the corresponding asymptotic solutions and their first derivatives at . Therefore after the matching, the integration constants are, and

 H =−12(p−1)evΩn12(p+1)+vΩn, A=1+He−vΩn, E =−e√α√α+2(2+2Aα(1−p)(p2−1)(p2+5)), B=1+Ee−√α+4Aα(p2−1)(p2+5), B =1+Ee−√α+4Aα(p2−1)(p2+5), F=e√β√β+3(−3+B−12(3−p)K), C =1+Fe−√β−B+K, G=e√β√β+23Aβn21(1−p)2(3p+8m−3), D =Ge−√β−3Aβn213p+8m−3, (47)

where , where  is the scalar quartic coupling.

## References

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