# Very light dilaton and naturally light Higgs boson

###### Abstract

We study very light dilaton, arising from a scale-invariant ultraviolet theory of the Higgs sector in the standard model of particle physics. Imposing the scale symmetry below the ultraviolet scale of the Higgs sector, we alleviate the fine-tuning problem associated with the Higgs mass. When the electroweak symmetry is spontaneously broken radiatively à la Coleman-Weinberg, the dilaton develops a vacuum expectation value away from the origin to give an extra contribution to the Higgs potential so that the Higgs mass becomes naturally around the electroweak scale. The ultraviolet scale of the Higgs sector can be therefore much higher than the electroweak scale, as the dilaton drives the Higgs mass to the electroweak scale. We also show that the light dilaton in this scenario is a good candidate for dark matter of mass , if the ultraviolet scale is about . Finally we propose a dilaton-assisted composite Higgs model to realize our scenario. In addition to the light dilaton the model predicts a heavy axial vector boson and two massive, oppositely charged, pseudo Nambu-Goldstone bosons, which might be accessible at LHC.

###### Keywords:

light dilaton, scale symmetry, composite Higgs, naturalness problem^{†}

^{†}institutetext: Department of Physics, Pusan National University, Busan 46241, Korea\arxivnumber

1703.05081 \preprintPNUTP-17/A01

## 1 Introduction

The standard model (SM) of particle physics, which has been very successful in describing the interactions of elementary particles, is finally completed by the discovery of its last missing piece, the Higgs particle, at the large hadron collider (LHC) Aad:2012tfa ; Chatrchyan:2012xdj . The properties of the Higgs particle are measured to be consistent with the standard model prediction, better than at the percent level by the subsequent experiments CMS:2017rli ; ATLAS:2017myr . But, nonetheless, the SM is widely regarded as an effective theory below the electroweak scale , set by the vacuum expectation value (vev) of Higgs fields. Since the SM does not have any obvious symmetry to protect the mass of Higgs particle, which is very sensitive to short distance physics, it needs to be highly fine-tuned, if the ultraviolet (UV) scale of Higgs physics is much higher than TeV 'tHooft:1979bh . New physics at TeV is hence currently actively explored at the LHC to find a hint for physics beyond the standard model, though no clear signals have been found yet.

While signals for new physics are actively being probed at LHC, the lower limit of new particle masses has been pushed up to almost at the Run 2 of LHC Aaboud:2017yyg ; CMS:2016crm , putting most models of physics beyond the standard model (BSM) such as walking technicolor, composite Higgs or supersymmetry in great tension with LHC. We might therefore need to seek alternative solutions to the naturalness problem of the standard model, one of the basic guiding principles for new physics. Recently there has been proposed an interesting mechanism to select the Higgs mass dynamically without introducing new physics at the electroweak scale Graham:2015cka . The idea is to construct a model that has many (or infinite) local minima for a wide range of a field that cosmologically relaxes into a local minimum at the electroweak scale, starting from a local minimum at the ultraviolet (UV) scale of the Higgs sector, to give a small mass of the electroweak scale to Higgs fields. The QCD axion fits this criterion, if it couples to the Higgs sector, since its potential is periodic under the shift symmetry to have infinitely many local minima, and hence the field is called relaxion.

In this paper we propose a very minimal model which assumes only very light dilaton in addition to the standard model particles up to a UV cutoff scale, , much higher than the electroweak scale. Our model provides the naturally light Higgs boson, though its UV scale is much higher than the electroweak scale. To discuss the mechanism for our model, we first assume that our model is an effective theory below the cutoff scale, . One possible candidate for the UV completion of our model, as discussed later, is a dilaton-assisted composite Higgs model, based on Banks-Zaks gauge theories with a quasi infrared (IR) fixed point Banks:1981nn , where both the Higgs boson and the dilaton are (composite) Nambu-Goldstone bosons from strong dynamics in UV, corresponding to the spontaneously-broken global symmetry Kaplan:1983fs and scale symmetry, respectively. Being a Nambu-Goldstone boson, associated with spontaneously-broken scale symmetry at the UV scale of the Higgs sector, the dilaton in our model does a similar role as relaxion that alleviates the naturalness problem of the standard model Higgs.

The standard model is scale invariant classically, if one turns off the Higgs mass or the relevant operators in the Higgs potential. In a classic paper Coleman:1973jx , however, Coleman and Weinberg (CW) showed that, even if one imposes the scale invariance at the quantum level in the Higgs sector of SM, the Higgs field could develop a vev to break the electroweak symmetry spontaneously by the radiative corrections. Since the value of Higgs vev is determined by the dimensional transmutation of the quartic coupling in the CW mechanism, it should be chosen by experiments; to account for the weak interactions. The standard model fermions and the weak gauge bosons get mass from the Higgs vev through the Yukawa and gauge couplings with the Higgs fields. The problem of CW mechanism is however that the Higgs mass turns out to be too small, compared to the experimental value, , unless one introduces extra bosons Dermisek:2013pta ; Hill:2014mqa . Furthermore, the standard model has to be fine-tuned from the intrinsic ultraviolet scales such as the Landau pole associated with the weak hypercharge to keep the scale invariance Bardeen:1995kv . Our model relies on the electroweak symmetry breaking à la Coleman-Weinberg but evades these problems by embedding the Higgs sector into an almost stable conformal sector at the UV scale of the standard model, which leads to a very light dilaton that generates additional contributions to the Higgs mass of the order of the Higgs vev, .

The ultraviolet theory of the Higgs sector in the standard model is assumed to be near conformal such as the gauge theories with the Banks-Zaks infrared (quasi) fixed point Banks:1981nn and the scale symmetry is spontaneously broken near the IR fixed point to generate a very light dilaton as a Nambu-Goldstone boson. The dilaton of the UV sector then drives the Higgs mass to a small value, controlled by the scale anomaly or the vacuum energy of the UV sector, once the Higgs field develops a vev. At low energy our model contains only the standard model with very light dilaton, which is therefore different from previous models Bardeen:1995kv ; Meissner:2006zh that attempt to solve the naturalness problem by imposing the scale invariance in the Higgs sector, not broken spontaneously. We also show that the light dilaton of our model abundantly constitutes the dark matter in our universe once it is non-thermally produced at early universe by the vacuum misalignment of the dilaton field. Finally we propose a specific dilaton-assisted composite Higgs model to realize our scenario that the very light dilaton derives the Higgs mass to the electroweak scale.

## 2 Very light dilaton and scale anomaly

The standard model (SM) of elementary particles is scale-invariant in the classical limit, if one turns off the Higgs mass term (and also the cosmological constant term, which we neglect in our discussions), but the scale symmetry is broken radiatively by quantum effects. Since our model assumes a spontaneously-broken scale symmetry in the UV theory of the Higgs sector, one is led at low energy to an extension of the standard model that still preserves the scale symmetry at the operator level up to the scale anomaly, though spontaneously broken.

### 2.1 Coleman-Weinberg potential.

We first review the (unsuccessful) scenario of Coleman and Weinberg Coleman:1973jx that Higgs field might be a dilaton in the standard model. CW showed that even if one imposes in the standard model the scale-invariance by taking the quadratic term in the Higgs effective potential to vanish

(1) |

the scale symmetry is spontaneously broken by radiative corrections. At one-loop, for instance, the Higgs field develops an effective potential to have a minimum away from the origin Coleman:1973jx ; Gildener:1976ih ,

(2) |

where and are the couplings of electroweak gauge interactions, respectively ^{1}^{1}1CW did not include top quark. If one includes the top quark, the effective potential changes its sign and the electroweak symmetry does not break. But, one could break it radiatively by introducing new heavy bosons that couple to Higgs fields Hill:2014mqa .. By expanding the potential around the minimum, one finds the Higgs mass to be
for and the weak gauge boson masses, and . The scale-invariant Coleman-Weinberg potential leads to too small Higgs mass, compared to the measured value, . Furthermore, if one includes the top quark, the one-loop effective potential changes its sign and the CW mechanism does not work. As we show however in our model, where the scale symmetry is spontaneously broken at the ultraviolet scale of the Higgs sector, a quadratic term in the Higgs potential is induced at the electroweak scale to generate the Higgs mass of the electroweak scale, when the dilaton develops a small vacuum expectation value, similar to the relaxion mechanism, provided that the CW mechanism works, having extra bosons Hill:2014mqa .

### 2.2 A model for light dilaton

Below the UV scale of the standard model, which we denote , taken to be much larger than , the Higgs potential is given as, neglecting possible irrelevant operators,

(3) |

where the quadratic term is not protected in general and naturally of order of the UV scale, .^{2}^{2}2In the composite Higgs model the quadratic term will be quite smaller than , since it is protected by the shift symmetry, broken only radiatively. Being parameters of the low-energy effective theory, the Higgs mass and the quartic coupling include all the ultraviolet contributions from the UV theory above the cutoff scale that are relevant at low energy. Especially the mass term includes the contributions from the massive modes in the UV theory or certain intrinsic scales of the UV sector such as the scale for the conformal phase transition in the case of conformal UV theories Tavares:2013dga .
In the case of the composite Higgs model, that we will focus on later as a possible model that realizes our mechanism, the Higgs mass is protected by the shift symmetry and generated by the Higgs interactions with the standard model particles such as top quark or EW gauge bosons, the mass term in eq. (3) then should be regarded as the counter term to the SM contributions to the Higgs mass that contains the effect of UV physics.

Since the scale symmetry is assumed to be spontaneously broken near the infrared fixed point of the UV theory like the Banks-Zaks theories, the symmetry breaking scale is much higher than the dynamical or infrared scale of the UV theory, , known as Miransky scaling Miransky:1996pd or Berezinskii-Kosterlitz-Thouless (BKT) scaling Berezinsky:1970fr ; Kosterlitz:1973xp . Our UV model is therefore almost scale-invariant for the wide range of scales, . (See figure 1.)

When the scale symmetry is spontaneously broken, the dilatation current creates a Nambu-Goldstone boson, the dilaton, denoted as , out of vacuum:

(4) |

where is the dilaton decay constant, and the dilatation current with the energy-momentum tensor that couples to gravity ^{3}^{3}3As supported by the Schwinger-Dyson analysis Hashimoto:2010nw , one can see that the dilaton decay constant should be the UV scale or not the IR scale, , that measures the strength of the scale anomaly, since the dilaton has to decouple from the theory if one takes ..
In order for the dilaton to behave like the relaxion, it has to couple to the Higgs fields. One natural way to achieve this is to assume that both the dilaton and the Higgs boson come from the same UV dynamics.
Being the low-energy effective theory of a scale-invariant UV theory of the Higgs sector, all the scale-symmetry violating terms in the Higgs sector are coupled to the dilaton field.
The (anomalous) Ward identity of the scale symmetry fixes how the dilaton couples to the Higgs fields:
Consider the following Green’s function,

(5) |

Upon integrating over all spacetime points, after taking the total divergence, one gets

(6) | |||||

(7) |

If one assumes the second term in eq. (7) is saturated at low energy by the dilaton, known as the hypothesis of partially conserved dilatation currents (PCDC), then one gets

(8) |

which shows that the strength to emit the dilaton by is as realized in the effective theory by , the first nontrivial term in the expansion of the nonlinear coupling of the dilaton to the quadratic Higgs fields, .

The Higgs sector of the standard model now becomes at low energy (), suppressing the Higgs couplings to fermions,

(9) |

where is the Higgs field and is the electroweak covariant derivative. The potential in the effective theory contains the scale anomaly term and the Higgs potential term with its coupling to the dilaton,

(10) |

We note that because the dilaton transforms nonlinearly under the scale transformation in the SM sector, , is scale invariant and the scale anomaly term changes accordingly, .^{4}^{4}4The anomalous Ward identity with and

The scale anomaly term in the potential is determined by the anomalous Ward identity of scale symmetry as Migdal:1982jp

(12) |

where is the vacuum energy density of the UV theory of the Higgs sector ^{5}^{5}5The vacuum energy in eq. (12), that contributes to the dilaton mass, is due to the vev of the order parameter of the scale symmetry, subtracting out the usual perturbative contributions, so that it vanishes when the vev vanishes Miransky:1989qc . and is the dilaton decay constant, .

The low energy theorem associated with the scale anomaly determines the dilaton mass, . As long as the scale symmetry is broken very close to the (quasi) infrared fixed point of the UV theory, there will be a large separation of two scales and , the dynamical (or infrared) scale of the (quasi) scale-invariant UV theory. We then have and the dilaton can be very light Choi:2011fy ; Choi:2012kx .

Since the UV completion of the Higgs sector is assumed to be (quasi) scale-invariant, one can impose the scale invariance at the cutoff scale on the standard model in the sense of Bardeen’s naturalness Bardeen:1995kv ^{6}^{6}6Our renormalization condition at the cutoff scale is technically different from that of Bardeen’s proposal.. We therefore choose the renormalization condition or the counter terms in eq. (10) such that the quadratic term of the Higgs field vanishes in the full 1PI effective potential Coleman:1973jx :

(13) |

This renormalization process is stable under any UV contributions because the very light dilaton, that coupled to Higgs fields, enjoys the shift symmetry, . (See more on this in appendix A.) The effective potential then becomes

(14) |

where is the Coleman-Weinberg potential for (massless) Higgs fields. At one-loop

(15) |

where is a constant, to be chosen such that , and is nothing but the one-loop beta function of the Higgs quartic coupling, , assumed to be positive by having extra bosons Hill:2014mqa . As the Higgs sector flows into the infrared, the Higgs field develops a vev by the CW mechanism Coleman:1973jx . As soon as the Higgs field gets a vev, it drives the minimum of the dilaton potential away from the origin, . When the Higgs field develops a vev, , it breaks the scale symmetry explicitly and the dilaton potential gets an additional contribution (See figure 2)

(16) |

where now depends on from the minimization of .

The dilaton field therefore develops a vev away from the origin. For the one-loop CW potential one finds

(17) |

where we have taken the vacuum energy, . The Higgs mass then becomes, neglecting small mixing with the dilaton,

(18) |

Since the dynamical scale or the infrared scale of the UV theory of the Higgs sector is assumed to be of order of , its vacuum energy , where the constant is given by the structure of the UV theory. In the case of Banks-Zaks gauge theories with a quasi IR fixed point, the constant depends only on the gauge group and the number of fermions Miransky:1989qc . Thus the Higgs mass is naturally given as the electroweak scale or .

In our model, therefore, having the scale-invariant UV theory of the Higgs sector, that gives the coupling between the dilaton and the Higgs boson, the dilaton dynamically relaxes the Higgs mass to the electroweak scale, giving the naturally light Higgs boson or . Without severe fine-tuning we have therefore dynamically raised the ultraviolet scale of the Higgs sector to be much higher than the electroweak scale, alleviating the naturalness problem associated with the Higgs mass. The scale symmetry does a crucial role in our mechanism. Having the very light dilaton at the UV scale , the Higgs sector is almost scale-invariant. The curvature of the Higgs potential, therefore, has to be chosen to vanish at the origin by the renormalization condition to be consistent with the scale symmetry, . However, once the Higgs sector flows into IR, the Higgs field develops a vev, by the CW mechanism, generating the IR scale. The Higgs vev therefore sets the scale for the Higgs mass.

## 3 Very light dilaton as dark matter

Besides the naturalness problem that we discussed, another strong motivation for physics beyond the standard model is to account for the dark matter that constitutes about 23% of the total energy of our present universe. According to the current standard big-bang cosmology, cold dark matter with a cosmological constant, so-called the CDM fits the current observations such as the cosmic microwave background (CMB) best Bennett:2012zja ; Ade:2013sjv . A very light dilaton has been shown to be one of the best candidates for the cold dark matter Choi:2011fy ; Choi:2012kx .

### 3.1 Life time

The dilaton couples to the standard model particles, once they get mass by the Higgs mechanism that breaks the electroweak symmetry. The light dilaton therefore decays into two photons through a loop process (and also into neutrinos and gravitons, which we neglect), as shown in figure 3.

The decay rate is given at one loop for the very light dilaton as

(19) |

where is approximately a constant times the electric charge squared, summed over all charged particles in the standard model. We estimate the lifetime of the dilaton

(20) |

In order for the dilaton to be long-lived to become a dark matter candidate of mass, with decay constant , the UV scale has to be by the low energy theorem for the dilaton, . If the dilaton decay constant is as high as the GUT scale, , the dilaton mass can be as low as . For , we have , if , or , if . Therefore, if the UV scale of SM is around , the dilaton mass is about .

### 3.2 Relic abundance of dilaton

Since the dilaton is weakly coupled, it will not be in thermal equilibrium with other particles in early universe, when it is produced. However, by the vacuum misalignment the light dilaton will be non-thermally produced in early universe. If we take the degree of the misalignment to be , the relic density of the dilaton will be at the time of oscillation from the misalignment

(21) |

Since the relic density at present is given as , where is the entropy density at temperature , we find the dilaton dark matter contributes to energy of our present universe as Choi:2011fy ; Choi:2012kx

(22) |

where is the effective degrees of freedom of early universe at the temperature for the coherent dilaton field starting to oscillate. Very light dilaton as dark matter has been studied in Choi:2011fy ; Choi:2012kx in the context of walking technicolor. The light dilaton in our model might be detected in similar experiments such as a microwave cavity experiment under strong magnetic fields.

## 4 Dilaton-assisted composite Higgs model

In this section we propose a specific model to realize our scenario that the dilaton relaxes the Higgs mass to the electroweak scale. This model is based on a composite Higgs model, where the Higgs boson is a pseudo Nambu-Golstone boson, associated a global symmetry, broken spontaneously by strong dynamics at Kaplan:1983fs ; Contino:2010rs . The Higgs mass is protected by the (approximate) shift symmetry that is radiatively broken by the electroweak interactions, giving the loop-suppressed Higgs mass,

(23) |

where is the coupling of the electroweak interactions. On top of these features of the composite Higgs, our model needs to exhibit a (quasi) IR fixed point to have a very light dilaton at low energy that couples to the Higgs fields.

Consider a composite Higgs model based on the gauge theory with Dirac fermions () of the fundamental representation Galloway:2010bp ; Cacciapaglia:2014uja and with Dirac fermions () in the symmetric second-rank ternsor representation Hong:2004td . Since the spinors are pseudo real in the gauge theory, the global symmetry is for (massless) Dirac fermions, which breaks down to , once the fermion bilinears form condensates Lewis:2011zb . The Higgs field is then identified as one of the Goldstone bosons living on the coset space, , where the SM gauge group is embedded in its unbroken subgroup, so that the Higgs fields transform correctly under the SM gauge symmetry.

To see whether our composite Higgs model is near the conformal window or not, we study the two-loop beta function of the gauge theory with fundamental Dirac fermions and Dirac fermions in the second-rank symmetric tensor representation, that is given as

(24) |

with the coefficient and , known as

(25) | |||||

(26) | |||||

The theory will be asymptotically free if and will have a IR fixed point near at , if and the chiral symmetry is unbroken. The chiral symmetry of the Dirac fermions will break at the critical couplings, and for the fermions in the fundamental representation and in the symmetric second-rank tensor, respectively, if they are smaller than the would-be IR fixed point . The critical couplings are given in the ladder approximation Cohen:1988sq ; Hong:1989zza as

(27) |

For the gauge theory with fundamental Dirac fermions the lattice results show that the theory is in the conformal window, flowing into a stable IR fixed point Leino:2015bfg . This is consistent with our two-loop beta function analysis, which shows that the critical coupling for the chiral symmetry breaking is bigger than the IR fixed point, . Let us consider another gauge theory in the conformal window; the gauge theory with Dirac fermions in the fundamental representation and Dirac fermion in the symmetric second-rank tensor representation. Since the critical couplings for both representations, and are larger than the IR fixed point, , the theory will be in the conformal window, according to the analysis based on the two-loop beta function. The theory will flow from the asymptotically free theory to the IR fixed point. The coupling never becomes strong enough to break the chiral symmetry. Now, we gauge half of the flavor of the fundamental Dirac fermions so that they become bi-fundamental under (See Table 1.).

For the bi-fundamental fermions () the attractive forces are additive and thus the critical couplings for the chiral symmetry breaking will be smaller than in the ladder approximation, since the Bethe-Salpeter Kernel for the fermion-bilinear in the scalar channel is approximately in the short-distance limit Hong:1989zza

(28) |

where is the coupling of at the symmetry breaking scale, , and is the distance square of the four-dimensional Euclidean space. However, unlike the gauge theory, the gauge coupling runs, becoming strong at low energy (). Therefore we tune to become close to the at so that the chiral symmetry of the bi-fundamental fermions breaks dynamically very near the IR fixed point of the gauge theory ^{7}^{7}7Since the bi-fundamental fermions are charged under both gauge groups, the -function will have mixings between two gauge couplings. At two-loop for , where . The mixing will shift in perturbation the value of to . However, since is at most 0.56 before the chiral symmetry breaking, the mixing does not change the IR fixed point much and thus negligible for our discussions. ^{8}^{8}8We note that by gauging partially the flavor symmetry of the gauge theory, as in our case, one can move most of the gauge theories in the conformal window to the broken phase very near the conformal window.. Once the bi-fundamental fermions get dynamical mass, they will decouple at low energy and the coupling becomes stronger and stronger to break the chiral symmetry of down to and we will have two extra Goldstone bosons, . By identifying the unbroken as
the , the Goldstone bosons are oppositely charged and get mass , where is the electric charge and is the scale for the chiral symmetry breaking.
As the gauge theory flows into the IR, the bi-fundamental fermions get condensed at , breaking the chiral symmetry near the (quasi) IR fixed point. The coupling of will show the walking behavior, since its beta function for the wide range of scales, shown in figure 4,

(29) |

where the dynamical (IR) scale is given by the Miransky or BKT scaling,

(30) |

We see that the dynamical scale can be arbitrarily small, compared the chiral symmetry breaking scale , if is close to the IR fixed point . Our composite Higgs model therefore is almost scale-invariant for energy and there should be a dilaton associated with spontaneous breaking of scale symmetry, when the bi-fundamental Dirac fermions get condensed at to break its global symmetry down to .

Since the vacuum manifold is five dimensional, there will be five Goldstone bosons.
If we embed the standard model gauge group into the unbroken subgroup , the five Goldstone bosons can be decomposed into one doublet, to become
the SM Higgs boson, and one real -odd singlet scalar Katz:2005au ; Gripaios:2009pe ; Cacciapaglia:2014uja . The broken generator associated with the singlet scalar is nothing but the axial fermion number of the bi-fundamental fermion . Assuming it is non-anomalous ^{9}^{9}9This is always made possible, if one introduces leptonic fields that are charged under but not under the UV gauge interactions. , we weakly gauge it so that the singlet is absorbed into the gauge boson. The gauge boson gets mass , with being the coupling, and decouples from the SM particles at low energy.

When the subgroup in the unbroken global symmetry is gauged, the electroweak interaction contributes to the vacuum energy, lifting the degeneracy of the vacuum manifold. The correction to the vacuum energy at the leading order in the electroweak coupling expansion is given as (See figure 5), after the renormalization,

(31) |

where is the electroweak gauge boson propagator and are the electroweak currents, denoted as in figure 5. The composite Higgs field is nonlinearly realized, with the decay constant, by the Pagels-Stokar formula Hashimoto:2010nw .

In addition to the SM gauge bosons, the SM fermions will contribute to the vacuum energy through the Yukawa interactions. To calculate, for instance, the top Yukawa contributions to the vacuum energy, one needs to calculate the two-point function of the composite operators or of the UV theory, denoted as the bullets in figure 5, that source or sink the top-quark mass term, connected by the top-quark propagators. The zero mode of the composite operator for the top quark should be correctly normalized to give the top Yukawa coupling, . ^{10}^{10}10The SM fermions are external to the composite Higgs dynamics. Unlike the gauge interactions, the Yukawa interaction of SM fermions will be absent in the composite Higgs, unless the interaction for the Yukawa couplings is incorporated in the UV theory to begin with. Here we assume that the Yukawa couplings are generated in the UV theory through the four-Fermi interactions between the SM fermions and the fermions in the UV theory of the composite Higgs, similar to the extended technicolor Dimopoulos:1979es ; Eichten:1979ah .

Expanding the vacuum energy of the composite Higgs due to the vacuum misalignment in powers of the Higgs fields, , one finds the Higgs effective potential at the scale becomes for

(32) |

where with . The one-loop beta-function for the Higgs quartic coupling is adjusted to be positive in the composite Higgs model. For instance, the gauge-boson contribution to the one-loop beta-function to the quartic coupling is given as

(33) |

which makes the beta-function as long as .

In the dilaton-assisted composite Higgs model the (one-loop) effective potential for the composite Higgs fields and the dilaton is given as

(34) |

where we have chosen the renormalization condition that is consistent with the scale symmetry Bardeen:1995kv ,

(35) |

To find the vacuum configuration we minimize the effective potential:

(36) |

which gives

(37) |

using the relation of the composite Higgs model. Neglecting the small mixing with the dilaton, the Higgs mass becomes

(38) |

Since in our composite Higgs model Miransky:1989qc , either or has to be or the coupling to give .

By coupling the Higgs sector to the light dilaton, we have shown that the Higgs mass is given by the IR scale, , not by the UV scale, . This seems mysterious but the scale symmetry is working behind. As the Higgs sector flows into IR, , the dilaton transforms to keep the renormalization condition (35) until the Higgs field gets the vev, which breaks the scale symmetry. Hence the UV scale of the composite Higgs can be arbitrarily high. The cosmological or phenomenological requirements on the dilaton mass and its decay constant, however, will constrain the scale of the model. In our model with the composite-Higgs gauge group, if we take for instance and , the dilaton decay constant to give the dilaton mass

(39) |

The dilaton of this mass range is shown to be a good candidate for the dark matter Choi:2011fy ; Choi:2012kx .

## 5 Discussions and conclusion

In this paper we propose a mechanism that very light dilaton naturally derives the Higgs mass to the electroweak scale, if the Higgs field gets the electroweak vev à la Coleman-Weinberg mechanism and couples to the light dilaton. The scale symmetry, associated with the light dilaton, does a crucial role in our mechanism that the Higgs mass is given by the Higgs vev, , the IR scale of the Higgs sector.

We then show that the dilaton-assisted composite Higgs model, based on the gauge theory with two Dirac fermions in the bi-fundamental representation and one in the symmetric tensor representation of , realizes our scenario. Both the dilaton and the composite Higgs are shown to arise as (pseudo) Nambu-Goldstone bosons, once the Dirac fermions in the bi-fundamental representation get condensed.
The standard model is then coupled through the very light dilaton to the quasi-conformal composite Higgs model at . By imposing the scale symmetry on the standard model, the naturalness problem of Higgs mass is alleviated to the UV scale, . When the electroweak symmetry is radiatively broken by the CW mechanism, the dilaton potential gets an extra contribution from the Higgs vev, which then drives the dilaton vev away from the origin.
The non-vanishing dilaton vev relaxes the Higgs mass naturally to be of the electroweak scale, as the vacuum energy or the scale anomaly of the scale-invariant UV theory of the Higgs sector is of the UV scale, ^{11}^{11}11Our mechanism that the light dilaton relaxes the Higgs mass from the UV scale to the IR scale, might be the manifestation of the -theorem in the conformal field theory, studied in Komargodski:2011vj . This needs to be investigated further..

At the electroweak scale, much below the UV scale, the model contains the standard model and only one extra particle, the very light dilaton, which is shown to be a good candidate for dark matter in the universe. If we take for instance the UV scale and the dilaton decay constant , the dilaton mass becomes , which is then long lived enough and abundantly produced by the vacuum misalignment to constitute dark matter in our universe.

Finally, the dilaton-assisted composite Higgs model predicts in addition to the very light dilaton a heavy (axial) vector boson of mass and two, oppositely charged, pseudo Nambu-Goldstone bosons (SM singlet) of mass . If the UV scale of our composite Higgs model is around a few , their mass will be a few TeV or so, accessible at LHC.

###### Acknowledgements.

The author thanks D. Bak, K. Y. Choi, G. Giudice, D. B. Kaplan, D. Kim, H. D. Kim, J. Serra, A. Strumia and A. Wulzer for useful comments and discussions. The author is also grateful to the CERN Theory group for the hospitality during his participation at the CERN-CKC TH institutes and visit to CERN, where part of this work was done. This research was supported by Basic Science Research Program through the National Research Foundation of Korea (NRF) funded by the Ministry of Education (NRF-2017R1D1A1B06033701).## Appendix A On the stability of the renormalization condition

In this appendix we show that the renormalization condition, imposed in eq. (14), that the Higgs quadratic term vanishes at the UV cutoff of the Higgs sector is natural and stable under any radiative corrections from the UV physics of the Higgs sector, if the Higgs sector is embedded into the scale-invariant theory that breaks the scale symmetry spontaneously, leading to very light dilaton at low energy.

### a.1 Scale anomaly and the dilation effective potential

In the theory, where the scale symmetry is spontaneously broken, very light dilaton of mass , arises as a Nambu-Goldstone boson, provided that the scale anomaly is much smaller than the scale of spontaneous breaking of the scale symmetry

(40) |

where is the dilatation current and the dilaton decay constant is of the order of the spontaneous scale-symmetry breaking scale. Then, at low energy , taking , one can write down the low-energy effective theory of dilaton that saturates the scale anomaly:

(41) |

where describes the small fluctuations around the asymetric vacuum,

(42) |

with at the vacuum.

The dilatation current in the dilaton effective theory is given as

(43) |

The scale anomaly then takes Schechter:1980ak , using the equations of motion for ,

(44) |

From eqs. (42) and (44) we get

(45) |

We note that the anomaly equation (44) does not fix the constant . But, our choice of the vacuum, , fixes . For the nonlinear realization of the dilatation symmetry we rewrite to get

(46) |

with .

### a.2 Dilaton and scale invariance of the Higgs sector

To solve the fine-tuning problem of Higgs mass, we embed the Higgs sector to a scale-invariant theory in UV. The UV theory is assumed to break the scale symmetry spontaneously, generating dynamically a condensate . The scale defines the intrinsic scale of the UV theory such as the dynamical mass in eq. (30) or the scale of phase transitions in Tavares:2013dga .

Integrating out all the modes above the dynamical scale in the Higgs UV sector, the low energy effective theory of the Higgs fields is given as, turning off all the SM interactions except the Higgs self interactions and the dilaton coupling,

(47) |

where the ellipsis denotes the higher order terms of , suppressed by powers of . Note that we have included in the effective theory the the dilaton coupling to the Higgs fields, as they come from the same UV dynamics, shown in section 2.2. All the effects above the UV cutoff, taken to be , of the Higgs sector are approximated in the effective theory by two relevant and marginal operators, namely the Higgs quadratic coupling, , and the Higgs quartic coupling, . Since the scale symmetry that protects the Higgs quadratic coupling is spontaneously broken, generating a scale , it should be of the order of or , if one integrates out all the heavy modes of .

Now we argue that, because of the scale symmetry that is spontaneously broken at low enegy, the Higgs quadratic coupling is unphysical just like the phase of nucleon mass in the coupling of pions to nucleons is unphysical because of the spontaneously-broken chiral symmetry^{12}^{12}12The intrinsic scale is also unphysical in this sense. The physical quantities are such as the ratio in eq. (30) and the intrinsic scale at the vacuum, , or the Higgs quadratic coupling at the vacuum, . We often do not specify to the physical scale, when there is no confusion, since we choose .. To see this, we integrate out the heavy modes further down to . Neglecting the logarithmic corrections to , the Higgs quadratic coupling becomes

(48) |

This change of the quadratic term can be compensated, if we shift the dilaton field as

(49) |

Under the scale transformation the dilaton potential has to change as

(50) |

where . In terms of the shifted dilaton field, with , the dilaton potential becomes

(51) |

This transformation of the dilaton potential can be easily seen if one notes under the scale transformation the scale anomaly transforms as with

(52) |

and the anomaly equation becomes

(53) |

while the vacuum energy of the ground state or is left invariant. We note also that the kinetic term in the effective dilaton Lagrangian (46) is kept properly normalized by the anomaly equation (44).

We see that because of the shift symmetry of the dilaton field the Higgs sector is scale-invariant up to the logarithmic violation through the constant and the quartic coupling . Hence, as long as the shift symmetry of the dilaton is good enough, the Higgs quadratic coupling should be unphysical. This property is not spoiled under any radiative corrections from the UV physics of the Higgs sector with spontaneously broken scale-symmetry, because one can always compensate the radiative corrections by shifting the dilaton field, as we have shown in this appendix A.2. The constraint on the Higgs mass, studied in Tavares:2013dga , therefore does not apply to our model that has light dilaton from the spontaneously broken scale-symmetry, noted also in Ghilencea:2016dsl .

### a.3 The renormalization condition

Now we turn on the SM interactions of the Higgs fields, which will break the scale symmetry that the Higgs-dilaton sector enjoys. From the effective potential (10) or the effective Lagrangian density (47) we calculate the one-particle irreducible (1PI) effective potential for the Higgs fields by integrating out all SM particles and possibly some new particles to get at one-loop, neglecting the higher order terms,

(54) |

where the loop momentum is cut off at and the effective potential is expanded in powers of with their coefficients and being functions of Higgs couplings to SM particles and also to new additional heavy particles that the UV sector of Higgs fields might have^{13}^{13}13If one applies strictly to our discussion Bardeen’s original proposal for the naturalness problem Bardeen:1995kv , the only consistent quadratic terms allowed in the radiative corrections in (54) are ones due to heavy particles associated with the UV sector of the Higgs fields, but not the one from the regulator. Here, for simplicity, without any confusion the correction stands collectively for all radiative corrections to the quadratic term that the effective theory receives. . Though the scale symmetry is explicitly broken by SM interactions, one can still impose the renormalization condition (13) that the Higgs quadratic term in the 1PI effective potential at vanishes by redefining the dilaton field with a suitable choice of :

(55) |

The choice of the renormalization condition, eq. (55) or eq. (13), is consistent with the scale symmetry that the Higgs-dilaton Lagrangian of eq. (47) enjoys and also with the fact that the Higgs quadratic term is protected above the intrinsic scale of the UV sector by the symmetry^{14}^{14}14One may argue that the renormalization condition (55) is not compatible with the UV theory of the Higgs sector that has some new massive particles or nonperturbative scale. But, we emphasize that what matters is whether or not one can maintain the renormalization condition at all orders in perturbation. . We emphasize that the choice of in eq. (55) is equivalent to the choice of the counter term in the Coleman-Weinberg potential, since the quadratic term represents the effects of the UV sector of Higgs fields. Therefore, if we fix the UV cutoff the Higgs sector to be , the intrinsic scale of the UV theory at vacuum is determined by the condition with

(56) |

We note that the renormalization condition eq. (56) holds for any cutoff because the Higgs quadratic term in the effective potential eq. (54) is scale-covariant: Under the scale transformation the dilaton field transforms and the quadratic term becomes

(57) |

This is equivalent to saying that the Callan-Symmanzik equation for the 1PI two-point function of Higgs fields in Fourier transforms becomes

(58) |

## References

- (1) G. Aad et al. [ATLAS Collaboration], Phys. Lett. B 716, 1 (2012) [arXiv:1207.7214 [hep-ex]].
- (2) S. Chatrchyan et al. [CMS Collaboration], Phys. Lett. B 716, 30 (2012) [arXiv:1207.7235 [hep-ex]].
- (3) CMS Collaboration [CMS Collaboration], CMS-PAS-HIG-16-040.
- (4) The ATLAS collaboration [ATLAS Collaboration], ATLAS-CONF-2017-045.
- (5) G. ’t Hooft, NATO Sci. Ser. B 59, 135 (1980).
- (6) M. Aaboud et al. [ATLAS Collaboration], [arXiv:1707.04147 [hep-ex]].
- (7) CMS Collaboration [CMS Collaboration], CMS-PAS-EXO-16-027.
- (8) P. W. Graham, D. E. Kaplan and S. Rajendran, Phys. Rev. Lett. 115, 221801 (2015).
- (9) T. Banks and A. Zaks, Nucl. Phys. B 196, 189 (1982).
- (10) D. B. Kaplan and H. Georgi, Phys. Lett. 136B, 183 (1984).
- (11) S. R. Coleman and E. J. Weinberg, Phys. Rev. D 7, 1888 (1973).
- (12) D. Chway, T. H. Jung, H. D. Kim and R. Dermisek, Phys. Rev. Lett. 113, no. 5, 051801 (2014) [arXiv:1308.0891 [hep-ph]].
- (13) C. T. Hill, Phys. Rev. D 89, 073003 (2014).
- (14) W. A. Bardeen, FERMILAB-CONF-95-391-T, C95-08-27.3.
- (15) K. A. Meissner and H. Nicolai, Phys. Lett. B 648, 312 (2007); R. Foot, A. Kobakhidze, K. L. McDonald and R. R. Volkas, Phys. Rev. D 77, 035006 (2008); M. Shaposhnikov and D. Zenhausern, Phys. Lett. B 671, 162 (2009); S. Iso, N. Okada and Y. Orikasa, Phys. Lett. B 676, 81 (2009); L. Alexander-Nunneley and A. Pilaftsis, JHEP 1009, 021 (2010); T. Hur and P. Ko, Phys. Rev. Lett. 106, 141802 (2011); A. Farzinnia, H. J. He and J. Ren, Phys. Lett. B 727, 141 (2013).
- (16) E. Gildener and S. Weinberg, Phys. Rev. D 13, 3333 (1976).
- (17) G. Marques Tavares, M. Schmaltz and W. Skiba, Phys. Rev. D 89, no. 1, 015009 (2014) [arXiv:1308.0025 [hep-ph]].
- (18) V. A. Miransky and K. Yamawaki, Phys. Rev. D 55, 5051 (1997) Erratum: [Phys. Rev. D 56, 3768 (1997)] [hep-th/9611142].
- (19) V. L. Berezinsky, Sov. Phys. JETP 32, 493 (1971) [Zh. Eksp. Teor. Fiz. 59, 907 (1971)].
- (20) J. M. Kosterlitz and D. J. Thouless, J. Phys. C 6, 1181 (1973).
- (21) M. Hashimoto and K. Yamawaki, Phys. Rev. D 83, 015008 (2011) [arXiv:1009.5482 [hep-ph]].
- (22) A. A. Migdal and M. A. Shifman, Phys. Lett. B 114, 445 (1982).
- (23) K. Y. Choi, D. K. Hong and S. Matsuzaki, Phys. Lett. B 706, 183 (2011).
- (24) K. Y. Choi, D. K. Hong and S. Matsuzaki, JHEP 1212, 059 (2012).
- (25) V. A. Miransky and V. P. Gusynin, Prog. Theor. Phys. 81, 426 (1989).
- (26) C. L. Bennett et al. [WMAP Collaboration], Astrophys. J. Suppl. 208, 20 (2013).
- (27) P. A. R. Ade et al. [Planck Collaboration], Astron. Astrophys. 571, A1 (2014).
- (28) See, for reviews, R. Contino, arXiv:1005.4269 [hep-ph]; G. Panico and A. Wulzer, Lect. Notes Phys. 913, pp.1 (2016) [arXiv:1506.01961 [hep-ph]].
- (29) J. Galloway, J. A. Evans, M. A. Luty and R. A. Tacchi, JHEP 1010, 086 (2010) [arXiv:1001.1361 [hep-ph]].
- (30) G. Cacciapaglia and F. Sannino, JHEP 1404, 111 (2014) [arXiv:1402.0233 [hep-ph]].
- (31) D. K. Hong, S. D. H. Hsu and F. Sannino, Phys. Lett. B 597, 89 (2004) [hep-ph/0406200].
- (32) R. Lewis, C. Pica and F. Sannino, Phys. Rev. D 85, 014504 (2012) [arXiv:1109.3513 [hep-ph]].
- (33) A. G. Cohen and H. Georgi, Nucl. Phys. B 314, 7 (1989).
- (34) D. K. Hong and S. G. Rajeev, Phys. Lett. B 240, 471 (1990).
- (35) V. Leino, T. Karavirta, J. Rantaharju, T. Rantalaiho, K. Rummukainen, J. M. Suorsa and K. Tuominen, PoS LATTICE 2015, 226 (2016) [arXiv:1511.03563 [hep-lat]].
- (36) E. Katz, A. E. Nelson and D. G. E. Walker, JHEP 0508, 074 (2005) [hep-ph/0504252].
- (37) B. Gripaios, A. Pomarol, F. Riva and J. Serra, JHEP 0904, 070 (2009) [arXiv:0902.1483 [hep-ph]].
- (38) S. Dimopoulos and L. Susskind, Nucl. Phys. B 155, 237 (1979).
- (39) E. Eichten and K. D. Lane, Phys. Lett. 90B, 125 (1980).
- (40) Z. Komargodski and A. Schwimmer, JHEP 1112, 099 (2011).
- (41) J. Schechter, Phys. Rev. D 21, 3393 (1980).
- (42) D. M. Ghilencea, Z. Lalak and P. Olszewski, Phys. Rev. D 96, no. 5, 055034 (2017) [arXiv:1612.09120 [hep-ph]].