Higgs Physics
Abstract
We discuss the interpretation of the LHC Higgs data and the test of the Higgs mechanism. This is done in a more modelindependent approach relying on an effective Lagrangian, as well as in specific models like composite Higgs models and supersymmetric extensions of the Standard Model. The proper interpretation of the data requires the inclusion of higherorder corrections both for the relevant Higgs parameters and the production and decay processes. We review recent results obtained within the Collaborative Research Centre / Transregio 9 “Computational Particle Physics”.
keywords:
Higgs physics, beyond the Standard Modelcompress
1 Introduction
With the announcement of the discovery of a new scalar particle by the LHC experiments ATLAS :2012gk () and CMS :2012gu () particle physics has entered a new era. The discovery immediately triggered activities to study the nature of this particle. The determination of its properties like the spin and parity quantum numbers and the couplings to other Standard Model (SM) particles strongly suggest it to be a Higgs boson, i.e. the particle responsible for electroweak symmetry breaking (EWSB). From the available data, however, it cannot be concluded yet that it is the SM Higgs boson. There is still room for interpretations within numerous extensions beyond the SM (BSM). At the same time, there is no hint for the existence of new particles that might shed light on the true nature of EWSB, which can be weakly or strongly interacting. In view of no direct observation of new states, an effective Lagrangian for the light boson is needed that parametrizes our ignorance of the EWSB sector. Such an effective description is valid as long as New Physics (NP) states appear at a scale much larger than the Higgs boson mass, .
At the LHC the Higgs boson couplings cannot be measured without applying modelassumptions. Only ratios of branching ratios, respectively, of couplings are accessible. In order to extract information on the Higgs boson couplings, fits are performed to the experimentally measured values of the signal strengths . The signal strengths quantify the Higgs signal rates in a specific final state with respect to the corresponding SM expectation, and hence are equal to one for the SM Higgs boson. The effective Lagrangian provides a tool that allows to consistently depart from the SM and to calculate BSM rates that can then be used in the fit to the values.
The ultimate step in the experimental verification of the Higgs sector is the measurement of the Higgs selfcouplings. With the experimentally extracted selfcouplings the Higgs potential can be reconstructed and its typical shape with a nonvanishing vacuum expectation value (VEV) can be tested. While the trilinear Higgs selfcoupling is accessible in Higgs pair production, the extraction of the quartic selfinteraction from triple Higgs production is beyond the scope of existing and future collider experiments. Due to the smallness of the double Higgs production cross sections and because of large backgrounds the extraction of the trilinear Higgs selfcoupling will be challenging and requires highestpossible energies and luminosities.
In this report we will review Higgs boson phenomenology at the LHC. We first investigate in Section 2 a general parametrization of BSM Higgs physics in terms of an effective Lagrangian approach and its implementation into automatic tools for the calculation of Higgs decay rates and production cross sections. Furthermore, its application in fits to the experimentally measured values will briefly be discussed. Section 3 is dedicated to the dominant Higgs pair production processes at the LHC and the higherorder corrections that we have calculated in order to improve the theoretical predictions. We give error estimates for the various processes and present the outcome of a parton level analysis in the gluon fusion process. The next two sections are devoted to Higgs interpretations in BSM models based on strong and weak interaction dynamics. In Section 4 we discuss the phenomenology of composite Higgs models as an example for strong EWSB. Section 5 is devoted to supersymmetric extensions of the Higgs sector, i.e. the minimal (MSSM) and NexttoMinimal Supersymmetric extension of the SM (NMSSM). The last section 6 closes the review by investigating Higgs coupling measurements at present and future colliders and what can be learned from these with respect to NP extensions beyond the SM.
2 Interpretation of LHC Higgs Data
The effective Lagrangian for the description of NP effects that emerge at scales far beyond the EWSB scale is based on an expansion in the number of fields and derivatives. Its detailed form depends on the assumptions that are applied. In view of the present LHC data it is reasonable to assume the Higgs to be CPeven and part of an doublet as well as baryon and lepton number conservation. The leading NP effects are then given by 53 operators with dimension 6 Burges:1983zg (); Leung:1984ni (); Buchmuller:1985jz (); Grzadkowski:2010es (), considering only one family of quarks and leptons. In case of CPviolation there are another 6 operators. In the stronglyinteracting light Higgs (SILH) basis the effective Lagrangian composed of the SM Lagrangian and the contributions from dimension6 operators is given by Giudice:2007fh (); Grinstein:2007iv ()
(1)  
The explicit form of and the Lagrangians containing the dimension6 operators, along with the conventions for the covariant derivatives and the gauge field strengths can be found in Ref. Contino:2013kra (). The Wilson coefficients are matrices in flavor space, and a summation over flavor indices has been implicitly assumed. Each of the operators is assumed to be flavoraligned with the corresponding mass term in order to avoid FlavorChanging Neutral Currents (FCNC) through the treelevel exchange of the Higgs boson. This leads to the coefficients being proportional to the identity matrix in flavor space. Assuming also CPinvariance they are taken to be real. Applying the power counting of Ref. Giudice:2007fh (), a naive estimate of the Wilson coefficients has been given in Contino:2013kra (). In the unitary gauge with canonically normalized fields, the SILH effective Lagrangian can be cast into the form
(2)  
Shown are terms with up to three fields and at least one Higgs boson. The couplings can be expressed as functions linear in the Wilson coefficients of the effective Lagrangian Eq. (1). The explicit relations can be found in Table 1 of Ref. Contino:2014aaa (). In particular, as a consequence of the accidental custodial invariance of the SILH Lagrangian at the dimension6 level Contino:2013kra () the following two relations hold
(3) 
A third relation, , holds if additionally custodial invariance is required for . Allowing for arbitrary values of the couplings , Eq. (2) is the most general effective Lagrangian at in a derivative expansion by focusing on cubic terms with at least one Higgs boson and making two further assumptions, which are CP conservation and vector fields that couple to conserved currents. The Higgs field in Eq. (2) needs not be part of an electroweak doublet, so that the Lagrangian can be considered as a generalization of . It contains 10 couplings involving a single Higgs boson and two gauge fields ( couplings, with ), 3 linear combinations of which vanish if custodial symmetry is imposed Contino:2013kra (). If the electroweak (EW) symmetry is realized nonlinearly, all Higgs couplings are independent of other parameters not involving the Higgs boson. In a linear realization, however, only 4 couplings are independent of the other EW measurements EliasMiro:2013mua (). Therefore in custodial invariant scenarios it is impossible, by focusing only on couplings, to tell whether the Higgs boson is part of an EW doublet. The doublet nature may be disproved by the decorrelation between the couplings and the other EW data Isidori:2013cga (); Brivio:2013pma (); Pomarol:2013zra (); Gupta:2014rxa ().
The parametrizations of BSM couplings in terms of the dimension6
extension given by as well as the one given by the
nonlinear Lagrangian Eq. (2) have been implemented in the
Fortran code Ehdecay^{1}^{1}1The program can be
downloaded at the URL:
http://wwwitp.particle.unikarlsruhe.de/ maggie/eHDECAY/.
Contino:2014aaa (). Furthermore two
benchmark composite Higgs models MCHM Agashe:2004rs () and
MCHM Contino:2006qr () have been included. It is based on the
code Hdecay Djouadi:1997yw (); Djouadi:2006bz () for the
computation of decay widths and branching ratios in the SM and the
minimal supersymmetric extension of the SM. All relevant QCD
corrections, which generally factorize with respect to the expansion
in the number of fields and derivatives of the effective Lagrangian,
have been included by using the existing SM computations. The
inclusion of the electroweak corrections in a consistent way is only possible in the
framework of the SILH Lagrangian and up to higher orders in . Here is
the weak scale GeV, and is given in terms of the NP scale and
the typical coupling of the NP sector. In Ehdecay the user can choose to take the EW corrections into
account in case of the SILH parametrization.
With the effective Lagrangian Eq. (2) at hand, the rates can be calculated by smoothly departing from the SM in a consistent way. The approach followed here at present LHCHiggsCrossSectionWorkingGroup:2012nn () is to assume that, while the couplings are modified by an overall modification factor, the coupling structures are not modified with respect to the SM.^{2}^{2}2The impact of higherdimensional operators on differential distributions, and the limitations of an effective Lagrangian approach have recently been discussed in Ref. Biekoetter:2014jwa (). Furthermore, the narrow width approximation is applied, factorizing the production and decay processes. Finally, the Higgs signal observed at the LHC is supposed to be built up by a single resonance. Our fits performed to the experimentally measured values Espinosa:2012ir (); Espinosa:2012im () show that the SM Higgs boson is compatible with the LHC Higgs data within 2. Our fits to a possible invisible branching ratio Espinosa:2012im (); Espinosa:2012vu () reveal that large invisible branching ratios are consistent with the LHC measurements.
3 Higgs Pair Production at the LHC
The measurements of the trilinear and quartic Higgs selfcouplings allow for the reconstruction of the Higgs potential Djouadi:1999gv (); Djouadi:1999rca () and thereby the experimental verification of its typical form with a nonvanishing VEV, required for the Higgs mechanism to work. Higgs pair production gives access to the trilinear Higgs selfcoupling. The dominant processes for double Higgs production at the LHC are:

the gluon fusion mechanism Eboli:1987dy (); Glover:1987nx (); Dicus:1988yh (); Plehn:1996wb ();

the fusion processes (VBF), () Eboli:1987dy (); Keung:1987nw (); Dicus:1987ez (); Dobrovolskaya:1990kx (); Abbasabadi:1988ja ();

the double Higgsstrahlung process, () Barger:1988jk ();

associated production of two Higgs bosons with a top quark pair, Moretti:2004wa ().
The loopinduced gluon fusion process provides the dominant contribution to Higgs pair production. It has been calculated at nexttoleading order (NLO) QCD in an effective field theory (EFT) approximation Plehn:1996wb () by applying the lowenergy theorem Ellis:1975ap (); Shifman:1979eb (); Kniehl:1995tn (), i.e. by assuming infinitely heavy quarks. The NLO cross section for a 125 GeV Higgs boson amounts to fb at a centerofmass (c.m.) energy of 14 TeV. In obtaining this number the leading order (LO) cross section has been calculated including the full mass dependence in order to improve the perturbative results. The NLO factor, i.e. the ratio between the NLO and the LO results is large and amounts to 1.52 depending on the c.m. energy. The error estimate based on the missing higher order corrections, PDF uncertainties and the application of the EFT approach results in an error of at 14 TeV Baglio:2012np (). In the meantime topquark mass effects at NLO have been estimated Grigo:2013rya (); Grigo:2013xya (); Maltoni:2014eza () and results at nexttonexttoleadingorder (NNLO) in the heavy top mass approximation deFlorian:2013uza (); deFlorian:2013jea (); Grigo:2014jma () are available.
The next important diHiggs production process is vector boson fusion into Higgs pairs, closely followed by Higgs pair production in association with a topquark pair, which is known at LO QCD only. For the VBF process we have calculated the NLO QCD corrections Baglio:2012np () in the structure function approach in complete analogy to the single Higgs VFB process Figy:2003nv (). Setting the renormalization and factorization scale equal to the momentum of the exchanged weak boson we found an increase of % of the total cross section with respect to the LO result. For the smallest diHiggs production process through Higgsstrahlung we have updated the NLO results in analogy to single Higgsstrahlung Altarelli:1979ub (); Han:1991ia (); KubarAndre:1978uy () and computed the QCD corrections at NNLO Baglio:2012np (). At NNLO there is a new gluoninitiated contribution to production to be taken into account. It turns out that in contrast to single Higgs production Dicus:1988yh (); Brein:2003wg (); Kniehl:1990iva (), its contribution at NNLO is sizeable.
Figure 1 shows the total LHC cross sections for the four classes of Higgs pair production as a function of the c.m. energy. The central renormalization and factorization scales, , respectively, , that have been used are ()
(4)  
where denotes the invariant mass of the Higgs pair. Note that all pair production cross sections are times smaller than the corresponding single Higgs production channels. High luminosities are therefore required to probe the Higgs pair production channels at the LHC. The smallness of the cross sections together with the large QCD backgrounds at the LHC make the analysis of diHiggs production challenging. We have performed a partonlevel analysis for the dominant gluon fusion process into Higgs pairs in different final states, which are , and with the bosons decaying leptonically. While the final state turns out not to be promising after applying acceptance and selection cuts, the significances in the and final states reach and , respectively, after applying the cuts. The event numbers are not too small so that they are promising enough to start a real experimental analysis taking into account detector and hadronization effects. The sensitivity of the various pair production processes to the trilinear Higgs coupling is diluted by additional diagrams to the processes that do not involve the Higgs selfinteraction. The sensitivity can be studied by varying the selfcoupling in terms of the SM trilinear coupling by a scale factor . The most sensitive channel turns out to be by far the VBF production mode. Taking into account theoretical and statistical uncertainties in the pair production channels the trilinear Higgs selfcoupling may be expected to be measured within a factor of two.
4 Composite Higgs Models
Composite Higgs Models are examples of models with a strong dynamics underlying EWSB. In these models a light Higgs boson arises as a pseudo NambuGoldstone boson from a stronglyinteracting sector Kaplan:1983fs (); Dimopoulos:1981xc (); Banks:1984gj (); Kaplan:1983sm (); Georgi:1984ef (); Georgi:1984af (); Dugan:1984hq (). This implies modified Higgs couplings with respect to the SM. In Ref. Giudice:2007fh () an effective lowenergy description of a Strongly Interacting Light Higgs boson has been given, which can be viewed as the first term of an expansion in , with the EWSB scale and the scale of the strong dynamics . This SILH Lagrangian can be used in the vicinity of the SM limit given by . Larger values of as e.g. the technicolor limit, , require a resummation of the series in . This is provided by explicit models built in fivedimensional warped space. In the Minimal Composite Higgs Models (MCHM) of Refs. Agashe:2004rs (); Contino:2006qr () the global symmetry is broken down at the scale to on the infrared brane and to the SM on the ultraviolet brane. The modifications of the Higgs couplings in these models can then be described by one single parameter, given by . The modification factor of the Higgs coupling to fermions depends on the representations of the bulk symmetry into which the fermions are embedded. In the model of Ref. Agashe:2004rs (), called , the fermions are in the spinorial representation of , in the model of Ref. Contino:2006qr () they are in the fundamental representation. The question of the generation of fermion masses in composite Higgs models is solved by the hypothesis of partial compositeness Kaplan:1991dc (); Contino:2006nn (). It assumes that the SM fermions, which are elementary, couple linearly to heavy states of the strong sector with the same quantum numbers, implying in particular the top quark to be largely composite. These couplings explicitly break the global symmetry of the strong sector. The Higgs potential is generated from loops of SM particles with EWSB triggered by the top loops which provide the dominant contribution. The Higgs selfcouplings therefore also depend on the representation of the fermions, and the Higgs boson mass is related to the fermion sector. It has been shown that a lowmass Higgs boson of GeV can naturally be accommodated only if the heavy quark partners are rather light, i.e. for masses below about 1 TeV, see Contino:2006qr (); Matsedonskyi:2012ym (); Redi:2012ha (); Panico:2012uw (); Pappadopulo:2013vca (); Marzocca:2012zn (); Pomarol:2012qf (). Phenomenologically the modified Higgs couplings to the SM particles change the Higgs production and decay rates Contino:2014aaa (); Espinosa:2010vn (). Another important consequence is the increase of the cross section for double Higgs production in vector boson fusion with the energy Giudice:2007fh (); Contino:2010mh (); Grober:2010yv (); Contino:2013gna (). Finally due to the coupling modifications, composite Higgs models are challenged by electroweak precision tests (EWPTs) Giudice:2007fh (); Agashe:2005dk (); Barbieri:2007bh (); Pomarol:2008bh (); Contino:2010rs (). The tension with the and parameters Peskin:1991sw () can be weakened through the contributions from new heavy fermions Lavoura:1992np (); Lodone:2008yy (); Gillioz:2008hs (); Anastasiou:2009rv (); Grojean:2013qca (); Gillioz:2013pba ().
So far we do not have any direct evidence for new BSM particles. Indirect information on heavy fermion partners could in principle also be obtained from Higgs physics. These new states would contribute to the loopinduced couplings of the Higgs boson to gluons and photons. It is also these couplings that are involved in the most sensitive Higgs search channels. The structure of these couplings can effectively be described by the LowEnergy Theorem (LET). In Gillioz:2012se () we have extended the theorem to take into account possible nonlinear Higgs interactions as well as new states resulting from a strong dynamics at the origin of the EWSB. The dominant Higgs production process at the LHC, gluon fusion, is mediated by a top loop with a subleading contribution from the bottom loop. In composite Higgs models with heavy colored fermions and sizable couplings to the Higgs boson, these new states give additional loop contributions that should be taken into account. It has been shown that in explicit constructions gluon fusion into a single Higgs boson, , computed in the LET approximation, is insensitive to the details of the heavy fermion spectrum Falkowski:2007hz (); Low:2010mr (); Azatov:2011qy (); Furlan:2011uq (). The cross section only depends on the ratio , but not on the couplings and the masses of the composite fermions. Although the top Yukawa coupling receives a correction due to the mixing with heavy resonances, which depends on the composite couplings, this contribution is exactly canceled by the loops of the extra fermions, so that the cross section only depends on . This holds both in models with partial compositeness and in Little Higgs theories. The gluon fusion cross section in the composite Higgs model can therefore be obtained from the SM result by simply multiplying the latter with the squared rescaling factor of the Yukawa couplings, that comes from the nonlinearity of the model. Every correction due to the fermionic resonances can be neglected. This insensitivity to the composite couplings, however, holds exactly only in the LET approximation. There are corrections due to finite fermion mass effects. The LET approximates the gluon fusion Higgs production rate very well, and it indeed turns out that these corrections are very small, even for large values of the compositeness parameter .
Another process mediated by colored fermion loops is double Higgs production through gluon fusion. In composite Higgs models the process is changed in two ways compared to the SM. First, there is a genuinely new contribution to the amplitude from a new coupling between two Higgs bosons and two fermions, which arises from the nonlinearity of the strong sector. In the SM limit this coupling vanishes. Second, the effects from the top partners in the loop have to be taken into account. They also give rise to a new box diagram that involves offdiagonal Yukawa couplings. These Yukawa couplings only involve the top quark and its charge 2/3 heavy composite partners. The diagrams contributing to the process are shown in Fig. 2. In Ref. Grober:2010yv () a first study on Higgs pair production in composite Higgs models was performed, neglecting top partners. It was found that the cross section can be significantly enhanced due to the new coupling. An explicit calculation of the diHiggs production cross section in the LET approximation shows that it is insensitive to composite couplings. The reason is a cancellation completely analogous to the single Higgs production case. The comparison with Ref. Grober:2010yv (), where the full top mass dependence was retained, shows that the LET underestimates the true result considerably, however.
In the SM it has been known that the limit approximates the full result only within 20% Plehn:1996wb (). Moreover it gives rise to incorrect kinematic distributions Baur:2002rb (). The same is observed in composite Higgs models, and in particular in MCHM the validity of the expansion gets even worse. This behaviour can be understood by looking at the expansion parameter. In single Higgs production this is and the series converges quickly. In double Higgs production, however, the expansion is performed in with the partonic c.m. energy squared which is not small, so that the expansion is not as good as in the single Higgs case. In MCHM the presence of the new triangle diagram containing the coupling, which contrary to the triangle diagram with the virtual Higgs boson exchange does not vanish for large , renders the convergence of the expansion even worse.
This shall be exemplified for an explicit composite Higgs model, MCHM, with extra fermionic resonances. It is based on the symmetry pattern . The additional local symmetry is introduced in order to correctly reproduce the fermion charges. The SM electroweak group is embedded into and the hypercharge is then given by Agashe:2004rs (); Contino:2006qr (). The vectorlike fermions introduced in the model have quantum numbers such that they can mix linearly with the SM fermions, the lefthanded doublet and righthanded singlet of the third generation and . At the same time they have ’protoYukawa’ interactions with the composite Higgs. The composite fermions are required to transform as a complete under . In this representation no dangerously large treelevel corrections to the coupling arise, provided a discrete symmetry exchanging the and factors is imposed Contino:2006qr (). Under a of decomposes as . The bidoublet is formed by the doublets and , while is a singlet under .
The strongest experimental constraints on the model come from the electroweak precision measurements at the pole mass at LEP. The modified Higgs couplings to and bosons induce logarithmically divergent contributions to the and parameters, which are cutoff by the mass of the first composite vector resonance Contino:2010rs (). Another BSM effect is the direct contribution of the vector and axialvector resonances to the parameter. Finally the top partners give loop contributions both to the parameter and the vertex Agashe:2005dk (); Lodone:2008yy (); Gillioz:2008hs (); Anastasiou:2009rv (). Figure 3 (left) from Ref. Gillioz:2012se () shows the points from a scan over the parameter range of the model after applying a test, which assesses the agreement of the model with the experimental data. These are the latest EW precision data (EWPD) at that time, and the constraint Group:2009qk () was applied, which also was the then most uptodate value. The results are displayed for the lefthanded compositeness angle versus the mass of the lightest top partner, for the compositeness parameter . The constraints on the parameter space from the EWPD can be significantly relaxed by extending the fermion sector of the model Anastasiou:2009rv (); Gillioz:2013pba ().
Further constraints are due to flavor physics. In composite Higgs models there arise generically fourfermion operators contributing to flavorchanging (FC) processes and to electric dipole moments. The constraints depend on the exact flavor structure of the model and can be avoided in case of minimal flavor violation (MFV) Redi:2011zi (). While both FC processes and electric dipole moments are inhibited in this case, the MFV assumption requires a large degree of compositeness also for light quarks, so that they have sizeable couplings to the strong sector resonances and lead to a different phenomenology Delaunay:2013iia (). Dijet searches put constraints on the up and down quarks ATLAS:2012pu (); Chatrchyan:2013muj (), while the second generation quarks are practically not constrained DaRold:2012sz (). An alternative approach is to treat the top quark differently than the light quarks Redi:2012uj (). The flavor bounds can still be satisfied, and since the first two generations are mostly elementary the constraints from EWPT and searches for compositeness are relaxed. In this case both the lefthanded and righthanded top can be composite. We do not assume a specific flavor model here. Additional discussions of flavor constraints on composite Higgs models can be found e.g. in Ref. Vignaroli:2012si ().
Another restriction of the model arises from direct searches for new vectorlike fermions by ATLAS and CMS. Based on the experimental results from the searches for pairproduced fermions with subsequent decay into the final states , and given in cmsfermsearch (); atlasfermsearch (); cdffermsearch (), exclusion limits from direct searches have been included in Figure 3 (left). As fermion pair production is a QCD process it only depends on the mass of the heavy fermion . The constraint in a specific final state then reads,
(5) 
where is the upper bound on the cross section, as given by the experiment for each value . The QCD pair production cross sections have been obtained at approximate NNLO Aliev:2010zk (). The points that pass the direct search limits from the 7 TeV run are shown in green in Fig. 3 (left). The orange points are tested by LHC8.
The gluon fusion cross section can be computed applying the LET and can be cast into the form
(6) 
This result is valid to all orders in . It depends purely on the Higgs nonlinearities and is independent of the details of the fermion spectrum. When retaining the full mass dependence on the other hand, corrections alter the cross section and are expected to be of the order of at most a few percent. This is confirmed by the full computation of the cross section taking into account the exact dependence on the fermion masses, as can be inferred from Fig. 3 (right).
The figure displays the cross section for single Higgs production through gluon fusion including new fermionic resonances, normalized to the SM cross section with the full top mass dependence, as a function of the mass of the lightest resonance. The QCD factors, i.e. the ratios between the QCD corrected cross section and the LO result, cancel out under the assumption that the higher order corrections are the same in both cases. In green are shown the points that pass the EWPTs, gray and orange points do not satisfy the collider bounds. The agreement between the full result and the prediction using the lowenergy theorem, shown by the black line, confirms that the cross section for single Higgs production is almost independent of the details of the spectrum and is fixed only by the value of . For heavy fermion partners the sensitivity to the composite couplings practically vanishes. The LET hence provides a very accurate cross section for single Higgs production for any spectrum of the heavy fermions. The figure furthermore shows that in the MCHM5 single Higgs production is suppressed compared to the SM for . This can be understood from the LET result given in Eq. (6).
Applying the LET to double Higgs production results in the partonic cross section
(7) 
where denotes the Fermi constant and the strong coupling constant evaluated at the scale . The amplitude in the limit of heavy loop particle masses at all orders in is given by
(8) 
As in single Higgs production the LET cross section for Higgs pair production is insensitive to the details of the heavy fermion spectrum and fixed uniquely by . In contrast to single Higgs production, for Higgs pair production the cross section is enhanced compared to the SM. In the SM Higgs pairs are produced through Higgs bosons coupling to gluons via triangle loops and boxes. The related amplitudes interfere destructively. In the MCHM5 the two contributions are modified by , and there is an additional diagram with the twoHiggs twofermion coupling proportional to , which can hence have order one effects and thus govern the total cross section.
Figure 4 shows the double Higgs production process normalized to the SM cross section as a function of the lightest top partner mass. The points result from a scan over the parameter range of the model. In the computation of the cross sections the full mass dependence of the loop particles has been taken into account. In the black solid line the full mass dependence on the top quark mass has been kept while the heavy fermion partners have been integrated out. The dashed line displays the result in the LET approximation, i.e. sending all loop particle masses to infinity. The color code is the same as in Fig. 3. The figure shows that there is a sizeable dependence of the cross section on the spectrum of the heavy fermions. We have . The LET cross section and the one in the limit of heavy partners on the other hand only depend on . However, the LET approximation considerably underestimates the full result. Note that in the figure the cross section is consistently normalized to the SM result for . The result in the limit of heavy partners and keeping the full top mass dependence on the other hand, overestimates the cross section for masses of the lightest fermion partner below about 1 TeV. This is the region that is compatible with a 125 GeV Higgs boson. For larger masses of the fermion partners, the cross section approaches the result retaining only the toploop contribution, as expected. Higherorder QCD corrections have not been taken into account in the figure. Due to the additional twoHiggs twofermion diagram and the box diagram with different loop particle masses they cannot be taken over from the SM. For heavy loop particle masses the corrections should not be too different from the SM case though, so that they approximately cancel out in the ratio of the cross sections.
So far we have only treated the case of composite top quarks. With the bottom quark being the nextheaviest quark a sizeable mixing with the strong sector can be expected also for the bottom quark. Due to the small bottom mass, the LET cannot be applied any more and the loopinduced Higgs couplings to gluons are expected to depend on the resonance structure of the strong sector, with significant implications for the Higgs phenomenology Gillioz:2013pba (); Azatov:2011qy (); Delaunay:2013iia (). The effects of composite bottom quarks on composite Higgs models and the LHC Higgs phenomenology can be studied by embedding the fermions in the 10. This is the smallest possible representation of that allows to include partial compositeness for the bottom quarks and at the same time is compatible with EWPTs by implementing custodial symmetry. The bottom quark mass is in this case not introduced at hoc any more but generated through the mixing with the strong sector. The 10 leads to a larger spectrum of new heavy fermions compared to the previous case with composite top quarks only. The new vectorlike fermions transform under the and are given by , , and with electric charge 2/3, , and with charge 1/3 and finally , and with charge 5/3. The model is strongly constrained by EWPTs, in particular there are oneloop contributions to the nonoblique corrections to the vertex due to the partial compositeness of the bottom quark. This coupling has been measured very precisely and agrees with the SM prediction at the subpercent level. It is safe from large corrections for the fermion embedding in the 10 representation, where belongs to a bidoublet of and the is enlarged to . The general formulae for the contributions of new bottom partners in the loop corrections to have been derived in Gillioz:2013pba () and can be applied to other models with similar particle content. In order to test the viability of the model a scan over its parameter space has been performed, setting the top and bottom quark masses to GeV and GeV, respectively, and the Higgs boson mass to GeV. A test is performed including the constraints from EWPD, and only those points have been retained that also fulfil Chatrchyan:2012ep (). The result is shown in Fig. 5 in the versus plane. The smallest values are obtained for . High values lead to large , corresponding to a compatibility with EWPTs at 99% confidence level (C.L.). The positive fermionic contributions to the parameter play an important role here for the compatibility as they drive back the value into the region in accordance with the EW precision data.
in  
Experiment  
ATLAS  0.105  8.06/9  0.90  0.096  12.34/10  1.23 
0.0  17.54/13  1.35  0.0  17.73/14  1.25  
CMS  0.057  5.22/10  0.52  0.055  6.36/11  0.58 
0.0  9.90/14  0.71  0.0  10.09/15  0.67 
The SM limit is obtained for and , where sets the scale for the top and bottom partner masses. Due to the restriction of the scan to TeV it is not contained in the plot.
The LHC Higgs search data put further constraints on the model. The inclusion of heavy bottom and top quarks leads to changes in the Higgs Yukawa couplings and new heavy fermions in the loopinduced production and decay processes. In particular, in contrast to the heavy top partner case, in the dominant gluon fusion production process due to the mixing with bottom partners the LET cannot be applied any more, so that the cross section now depends on the details of the model. Also the compatibility with the direct searches for new vectorlike fermions performed by ATLAS atlassearch () and CMS cmssearch1 (); Chatrchyan:2013uxa () has to be tested. Flavor physics further constrains the model. As this depends on the exact flavor structure of the model which is not specified here, these constraints are not taken into account in this investigation. For a random scan over the parameter range a test is performed taking into account EWPTs, Higgs data and the experimental results on . The results from direct fermion searches are taken into account by discarding all points that lead to masses below the exclusion limits. In Table 1 the values of the best fit points are reported together with those for the SM for comparison. The constraint from has been included in two different ways. Either all points with are rejected or the best fit value given by the experiments is included in the test. The global is increased when including , in particular in the composite Higgs model. The table shows that the CMS CMSdata () data are better described than the ATLAS data ATLASdata (). The best fit points are obtained for for ATLAS and for for CMS. In the composite Higgs model their is slightly smaller than in the SM, due to the larger number of free parameters. An estimate of the relative goodness of the fit is given by , where denotes the number of degrees of freedom.
Our discussion shows that composite Higgs models, although challenged by constraints from EWPTs, flavor physics, direct searches for new fermions and the light Higgs mass, are still viable extensions beyond the SM Higgs. They provide an explanation of EWSB based on strong dynamics and hence an alternative to weakly coupled models as e.g. supersymmetry, which shall be discussed in the following.
5 Supersymmetric Higgs Models
Supersymmetric theories Volkov:1973ix (); Wess:1974tw (); Fayet:1976et (); Fayet:1976cr (); Fayet:1977yc (); Fayet:1979sa (); Farrar:1978xj (); Witten:1981nf (); Nilles:1983ge (); Haber:1984rc (); Sohnius:1985qm (); Gunion:1984yn (); Lahanas:1986uc (); Dimopoulos:1981zb (); Sakai:1981gr () provide a natural solution to the hierarchy problem by introducing a new symmetry between fermionic and bosonic degrees of freedom. They are among the most extensively studied BSM extensions. In order to ensure supersymmetry (SUSY) and an anomalyfree theory two complex Higgs doublets have to be introduced, to provide masses to the uptype fermions, and to ensure masses for the downtype fermions. In sections 5.1 and 5.2 we will discuss Higgs physics in two popular supersymmetric models, the minimal (MSSM) mssm () and nexttominimal supersymmetric model (NMSSM) nmssm (), respectively.
5.1 Associated heavy quark Higgs production in the MSSM
After electroweak symmetry breaking, three of the eight degrees of freedom contained in and are absorbed by the and gauge bosons, leaving five elementary Higgs particles in the MSSM. These consist of two CPeven neutral (scalar) particles , one CPodd neutral (pseudoscalar) particle , and two charged bosons . At leading order the MSSM Higgs sector is fixed by two independent input parameters which are usually chosen as the pseudoscalar Higgs mass and , the ratio of the vacuum expectation values of and , respectively. Including the oneloop and dominant twoloop corrections the upper bound of the light scalar Higgs mass is GeV mssmrad () for supersymmetric mass scales up to about a TeV.
An important property of the bottom Yukawa couplings is their enhancement for large values of . The top Yukawa couplings, on the other hand, are suppressed for large schladming (), unless the light (heavy) scalar Higgs mass is close to its upper (lower) bound, where their couplings become SMlike. The couplings of the various neutral MSSM Higgs bosons to fermions and gauge bosons, normalized to the SM Higgs couplings, are listed in Table 2, where the angle denotes the mixing angle of the scalar Higgs bosons .
SM  1  1  1  

MSSM  
0 
The negative direct searches for neutral MSSM Higgs bosons at LEP2 have lead to lower bounds of GeV and GeV lep2 (). The LEP2 results also exclude the range in the MSSM, assuming a SUSY scale TeV lep2 (). MSSM Higgsboson searches have continued at the collider Tevatron, see e.g. Aaltonen:2012zh (), and form the central part of the current and future physics program of the LHC atlas_cms_tdrs (). The present LHC searches at 7 and 8 TeV c.m. energy have excluded parts of the MSSM parameter space for large values of lhcmssm (). However, the recent discovery of a resonance with a mass near 125 GeV :2012gk (); :2012gu () is a clear indication for the existence of a SM or beyondtheSM Higgs boson. While the properties of the new particle, as determined so far, are consistent with those predicted within the SM, the bosonic state at 125 GeV can also be interpreted as a supersymmetric Higgs boson.
Neutral MSSM Higgs boson production at the LHC is dominated by gluon fusion, , and by the associated production of a Higgs boson with bottom quarks. Gluon fusion is most significant at small and moderate . At large values of , however, bottom–Higgs associated production
(9) 
constitutes the dominant Higgsboson production process. Here, we shall focus on precision calculations for bottom–Higgs associated production at the LHC. We refer the reader to Refs. Dittmaier:2011ti (); Dittmaier:2012vm (); Heinemeyer:2013tqa () and references therein for a discussion of higherorder calculations for gluon fusion.
The NLO QCD corrections to Higgsbottom associated production, Eq. (9), can be inferred from the analogous calculation involving top quarks tthnlo (); tthnlo2 (). However, they turn out to be numerically enhanced bbhnlo () by large logarithmic contributions from the phase space region with finalstate bottom quarks at small small transverse momenta. Those logarithms can be resummed by introducing bottomquark densities in the proton Barnett:1987jw () and by applying the standard DGLAP evolution. In this socalled fiveflavor scheme (5FS) the leadingorder process is bbh5lo ()
where the transverse momenta of the incoming bottom quarks, their masses, and their offshellness are neglected at LO. The NLO bbh5nlo () and NNLO bbh5nnlo () QCD corrections as well as the SUSY–electroweak corrections bbh5elw () to these bottominitiated processes have been calculated. They are of moderate size, if the running bottom Yukawa coupling is introduced at the scale of the corresponding Higgsboson mass. The fully exclusive process, calculated with four active parton flavors in a fourflavor scheme (4FS), and the 5FS calculation converge at higher perturbative orders, and there is fair numerical agreement between the NLO 4FS and NNLO 5FS cross section predictions Dittmaier:2011ti (); Dittmaier:2012vm (); bbhnlo (); bbhscale (). In Ref. Harlander:2011aa () a scheme has been proposed to match the 4FS and 5FS cross sections (“Santander matching”). The scheme is based on the observation that the 4FS and 5FS calculations of the cross section are better motivated in the asymptotic limits of small and large Higgs masses, respectively, and combines the two approaches in such a way that they are given variable weight, depending on the value of the Higgsboson mass.
If both bottom jets accompanying the Higgs boson in the final state are tagged, one has to rely on the fully exclusive calculation for . For the case of a single tag in the final state the corresponding calculation in the 5FS starts from the process with the finalstate bottom quark carrying finite transverse momentum. The NLO QCD, electroweak, and NLO SUSYQCD corrections to this process have been calculated bh5elw ().
Stateoftheart predictions as well as estimates of the corresponding parametric and theoretical uncertainties have been provided by the LHC Higgs Cross Section Working Group both for total Dittmaier:2011ti () and differential Dittmaier:2012vm (); Heinemeyer:2013tqa () cross sections.
Recently, the 4FS calculations for heavy quark plus Higgs associated production at the LHC have been improved by including the full SUSYQCD corrections within the MSSM and separating the dominating universal part in terms of effective Yukawa couplings Dittmaier:2014sva (). The SUSY loop corrections modify the treelevel relation between the bottom mass and its Yukawa coupling, which is enhanced at large deltab (). These corrections can be summed to all orders by replacing the bottom Yukawa coupling coefficients of Table 2 by Carena:1999py (); Guasch:2003cv ()
(10) 
where
(11)  
with . Here, are the sbottom mass eigenstates, and denotes the gluino mass.
To discuss the various contributions to the NLO SUSYQCD corrections, we focus on production as an example, and write the NLO cross section as
(12) 
where denotes the LO cross section evaluated with LO and PDFs, with the Yukawa coupling parametrized in terms of the running bquark mass , but without resummation of the enhanced terms. The correction comprises the enhanced terms according to Eq. (10), including their resummation. The remainder of the genuine SUSYQCD corrections is denoted by .
The total cross section for scalar Higgsboson radiation off bottom quarks at the LHC ( TeV) is shown in Fig. 6 for the MSSM benchmark scenario SPS1b snowmass () with . The fourflavor MSTW2008 pdfs mstw4 () have been used. In Table 3 we show the individual contributions to the NLO cross section.
[GeV]  

100  113.9  0.27  
200  200  0.39  
7 TeV  300  300  0.47  
400  400  0.53  
500  500  0.59  
100  113.9  0.17  
200  200  0.29  
14 TeV  300  300  0.39  
400  400  0.45  
500  500  0.49 
The pure QCD corrections , the enhanced SUSYQCD corrections , and the remainders of the SUSYQCD corrections are defined according to Eq. (12). The moderate NLO corrections in this MSSM scenario result from a compensation of the large, positive QCD corrections and large, negative SUSYQCD corrections. The smallness of the SUSYQCD remainder shows that the full NLO SUSYQCD corrections are approximated extremely well by the enhanced terms.
Let us briefly comment on heavy charged Higgs production at the LHC,
(13) 
In a twoHiggs doublet model of type II, like the minimal supersymmetric extension of the SM, the Yukawa coupling of the charged Higgs boson to a top quark and bottom antiquark is given by
(14) 
where is the Higgs vacuum expectation value in the SM, with the Fermi constant , and are the chirality projectors.
As in the case of neutral Higgs production with bottom quarks, the cross section for can be calculated in the four or fiveflavor schemes. Nexttoleading order predictions for heavy charged Higgs boson production at the LHC in a typeII twoHiggsdoublet model have been made in the past in both 5F Zhu:2001nt (); Gao:2002is (); Plehn:2002vy (); Berger:2003sm (); Kidonakis:2005hc (); Weydert:2009vr () and 4F schemes Peng:2006wv (); Dittmaier:2009np (), including also electroweak corrections Beccaria:2009my (); Nhung:2012er (). In Ref. Flechl:2014wfa (), the NLOQCD predictions have recently been updated and improved by adopting a dynamical scale setting procedure for the 5FS Maltoni:2012pa (). A thorough account of all sources of theoretical uncertainties has been given, and a Santandermatched prediction Harlander:2011aa () for the four and fiveflavor scheme calculations has been provided. Reference Flechl:2014wfa () also includes results for a wide range of , which allows the comparison between theory and experiment for a large class of beyondtheSM scenarios.
The cross section and uncertainty for the results of the 4F and 5F scheme calculations and their combination for TeV are presented in Fig. 7. The dynamical choice of the factorisation scale in the fiveflavor scheme calculation significantly improves the agreement between the four and fiveflavor schemes. The overall uncertainty of the matched crosssection prediction is approximately 20–30%, and includes the dependence on the renormalisation scale, the factorisation scale, the scale of the running bottom quark mass in the Yukawa coupling, as well as the input parameter uncertainties in the parton distribution functions, in the QCD coupling , and in the bottom quark mass.
5.2 Higgs Bosons in the NMSSM
The NMSSM nmssm () extends the Higgs sector by an additional singlet superfield . This entails seven Higgs bosons after EWSB, which in the limit of the real NMSSM can be divided into three neutral purely CPeven, two neutral purely CPodd and two charged Higgs bosons, and in total leads to five neutralinos. The NMSSM allows for the dynamical solution of the problem Kim:1983dt () through the scalar component of the singlet field acquiring a nonvanishing vacuum expectation value. Furthermore, the treelevel mass value of the lightest Higgs boson is increased by new contributions to the quartic coupling so that the radiative corrections necessary to shift the Higgs mass to GeV are less important than in the MSSM allowing for lighter stop masses and/or mixing and in turn less finetuning. The singlet admixture in the Higgs mass eigenstates entails reduced couplings to the SM particles. Together with the enlarged Higgs sector this leads to a plethora of interesting phenomenological scenarios and signatures. It is obvious that on the theoretical side the reliable interpretation of such BSM signatures and the disentanglement of different SUSY scenarios as well as their distinction from the SM situation require precise predictions of the SUSY parameters such as masses and Higgs couplings to other Higgs bosons including higherorder corrections. For the CPconserving NMSSM the mass corrections are available at oneloop accuracy Ellwanger:1993hn (); Elliott:1993ex (); Elliott:1993uc (); Elliott:1993bs (); Pandita:1993hx (); Ellwanger:2005fh (); Degrassi:2009yq (); Staub:2010ty (); Ender:2011qh (), and two loop results of O() in the approximation of zero external momentum have been given in Ref. Degrassi:2009yq (). Recently, first corrections beyond order O() have been given in Goodsell:2014pla (). In the complex case the oneloop corrections to the Higgs masses have been given in Ham:2001kf (); Ham:2007mt (); Ham:2001wt (); Ham:2003jf (); Funakubo:2004ka (); Graf:2012hh () with the logarithmically enhanced twoloop effects presented in Cheung:2010ba (). Quite recently we have provided the twoloop corrections to the Higgs boson masses of the CPviolating NMSSM in the Feynman diagrammatic approach with vanishing external momentum at O() Muhlleitner:2014vsa (). Higherorder corrections to the trilinear Higgs selfcoupling of the neutral NMSSM Higgs bosons have been provided in Nhung:2013lpa ().
In the following the implications of the loop corrections in the real and complex NMSSM to the Higgs boson masses, and for the CPconserving NMSSM, to the trilinear Higgs selfcouplings shall be presented. To set up the notation the NMSSM Higgs sector is briefly discussed. The Higgs mass matrix is derived from the NMSSM Higgs potential, which is obtained from the superpotential, the soft SUSY breaking terms and from the term contributions. Denoting the Higgs doublet superfields, which couple to the up and downtype quarks, by and , respectively, and the singlet superfield by , the scale invariant NMSSM superpotential is given by
(15) 
with the indices and the totally antisymmetric tensor . While the dimensionless parameters and can be complex in general, in case of CPconservation they are taken to be real. In terms of the quark and lepton superfields and their charge conjugates, indicated by the superscript , , the MSSM superpotential reads
(16)  
where the flavor and generation indices have been suppressed. In general the Yukawa couplings and in the MSSM superpotential Eq. (16) are complex. Neglecting generation mixing, their phases can be reabsorbed by redefining the quark fields. The MSSM term as well as the tadpole and bilinear terms of are assumed to be zero. With the Higgs doublet and singlet component fields , and , the soft SUSY breaking NMSSM Lagrangian is given by
(17)  
where denotes the soft SUSY breaking MSSM Lagrangian,
(18)  
Here , () and are the gaugino fields, and , , where the tilde indicates the scalar components of the corresponding quark and lepton superfields. In the soft SUSY breaking NMSSM Lagrangian Eq. (17) the soft SUSY breaking mass parameters of the scalar fields are real. The soft SUSY breaking trilinear couplings () and the gaugino mass parameters and , however, are complex in general but real in the CPconserving case. Here, furthermore squark and slepton mixing between the generations is neglected and soft SUSY breaking terms linear and quadratic in the singlet field are set to zero. In the expansion of the Higgs boson fields about the VEVs two further phases, and , appear,
(19) 
describing the phase differences between the three VEVs , and . For phase values , , the fields and () are the pure CPeven and CPodd parts of the neutral entries of , and . Exploiting the freedom in the phase choice of the Yukawa couplings to set and assuming the downtype and charged leptontype Yukawa couplings to be real, the quark and lepton mass terms yield real masses without any further phase transformation of the corresponding fields. Expansion about the VEVs leads to the Higgs boson mass matrix that can be read off from the bilinear neutral Higgs field terms in the Higgs potential. CPviolation introduces a mixing between CPeven and CPodd component fields, leading to a matrix in the basis , which can be expressed in terms of three matrices and ,
(20) 
where and are symmetric matrices, describing the mixing among the CPeven components of the Higgs doublet and singlet fields and among the CPodd components, respectively. In the CPconserving case the matrix , which mixes CPeven and CPodd components, vanishes. Due to the minimization conditions of the Higgs potential (),
(21) 
in the treelevel Higgs sector only one linearly independent phase combination appears after applying the tadpole conditions for and ,
(22) 
The tadpole condition for does not lead to a new linearly independent condition. Hence the CP mixing due to is governed by at treelevel. In the real case, the CPodd tadpole conditions vanish and are thus automatically fulfilled.
In order to obtain the mass eigenstates first the rotation matrix is applied to separate the wouldbe Goldstone boson field and then the matrix to rotate to the mass eigenstates (), yielding a diagonal mass matrix squared,
(23)  
(24) 
with and the superscript indicating treelevel masses. In the CPconserving case the mass matrix decomposes into Higgs mass matrices squared for the CPeven and CPodd component Higgs fields, and , respectively. The squared mass matrix is diagonalized through a rotation , yielding the CPeven mass eigenstates (),
(25)  
(26) 
The mass eigenstates are ordered by ascending mass, , where the superscript indicates the treelevel mass values. In the CPodd Higgs sector a first rotation is applied to separate the massless Goldstone boson , followed by a rotation to obtain the mass eigenstates (), cf. Ender:2011qh (),
(27)  
(28) 
The parameters of the treelevel Higgs potential in the CPviolating NMSSM are
(29) 
Some of the parameters are traded for more physical ones leading to the following parameter set