DESY 15-029

Neutral Higgs production at proton colliders

in the CP-conserving NMSSM

Stefan Liebler

DESY, Notkestraße 85,

22607 Hamburg, Germany

^{0}^{0}0e-mail address:
^{0}^{0}0stefan.liebler@desy.de

We discuss neutral Higgs boson production through gluon fusion and bottom-quark annihilation in the CP-conserving -invariant Next-to-Minimal Supersymmetric Standard Model (NMSSM) at proton colliders. For gluon fusion we adapt well-known asymptotic expansions in supersymmetric particles for the inclusion of next-to-leading order contributions of squarks and gluinos from the Minimal Supersymmetric Standard Model (MSSM) and include electroweak corrections involving light quarks. Together with the resummation of higher-order sbottom contributions in the bottom-quark Yukawa coupling for both production processes we thus present accurate cross section predictions implemented in a new release of the code SusHi. We elaborate on the new features of an additional SU singlet in the production of CP-even and -odd Higgs bosons with respect to the MSSM and include a short discussion of theoretical uncertainties.

## 1 Introduction

After the discovery of a scalar boson at the Large Hadron Collider (LHC) [1, 2] in 2012 an essential task of particle physicists is to reveal the nature of the Higgs-like state and thus the nature of electroweak symmetry breaking. Apart from deviations from the Standard Model (SM) prediction of the properties of the found Higgs-like state, further work includes the search for additional less and/or more massive scalar bosons, which can nicely be accommodated in supersymmetric models. The Next-to-Minimal Supersymmetric Standard Model (NMSSM) extends the Minimal Supersymmetric Standard Model (MSSM) by an SU singlet and allows the dynamical generation of the -term through electroweak symmetry breaking [3, 4]. The latter singlet-doublet mixing term in the superpotential lifts the MSSM tree-level upper bound of the Higgs mass given by the -boson mass. Thus, the NMSSM can easily accommodate the SM-like Higgs boson with a mass close to GeV. Whereas for the calculation of the NMSSM Higgs spectrum and branching ratios various spectrum generators are available and include higher orders in perturbation theory (see Section 3), the calculation of neutral Higgs production cross sections did not exceed leading order (LO) in quantum chromodynamics involving squarks and gluinos (SQCD) [5] and did not include electroweak corrections - apart from private implementations in e.g. HIGLU [6].

It is therefore timely to present the missing ingredients and a code for the calculation of accurate neutral Higgs production cross sections in the NMSSM, where the five neutral Higgs bosons are predominantly generated through gluon fusion and bottom-quark annihilation at a proton collider. For this purpose we extend the code SusHi [7]. For the time being we restrict our implementation to the real NMSSM without additional CP violation, such that CP-even and and CP-odd Higgs bosons and can be distinguished in the Higgs sector. Most recent efforts related to Higgs physics at the LHC are summarized in the reports of the LHC Higgs cross section working group [8, 9, 10]. The SM Higgs is mainly produced through gluon fusion, where the Higgs-gluon coupling is mediated through virtual top- and bottom-quarks [11]. Higher order QCD corrections at next-to-leading order (NLO) are of large importance [12, 13, 14]. In the effective theory of a heavy top-quark the inclusive cross section is known to next-to-next-to-leading order (NNLO) in QCD [15, 16, 17], in addition finite top-quark mass effects at NNLO were calculated [18, 19, 20, 21, 22]. Beyond NNLO QCD effects are accessible through resummation [23, 24, 25, 26, 27, 28] and electroweak corrections are known [29, 30, 31]. Meanwhile next-to-NNLO (NNNLO) QCD contributions were estimated in the so-called threshold expansion [32, 33, 34, 35], but they are not further considered in this publication.

The SM results for Higgs production through gluon fusion can be adjusted to the MSSM and the NMSSM through a proper reweighting of the Higgs couplings to quarks. However, the gluon fusion process can also be mediated through their superpartners, the squarks. With respect to the MSSM the only generically new ingredient, which goes beyond the projection of the physical Higgs bosons onto the neutral components of the two Higgs doublets, are couplings of the NMSSM singlet to squarks, since no couplings of the singlet to quarks or gauge bosons are present in the tree-level Lagrangian. It is therefore of importance to include squark contributions to gluon fusion at the highest order possible, even though they decrease in size with increasing squark masses. For the pseudoscalars squark contributions to gluon fusion are only induced at NLO, which motivates to go beyond just LO squark contributions for all Higgs bosons. For this purpose we adapt the works of Refs. [36, 37, 38] for the MSSM to present NLO SQCD contributions for the NMSSM, which are based on an expansion in terms of heavy supersymmetric particles taking into account terms up to ), ), ) and ), where denotes the Higgs mass and a generic SUSY mass. In contrast to the MSSM we are at present only working in this expansion of inverse SUSY masses and do not include an expansion in the so-called VHML, the vanishing Higgs mass limit () for the SQCD contributions, as implemented in evalcsusy [39, 40, 41] or discussed in Ref. [42]. In the latter limit higher-order stop-induced contributions up to NNLO level are known [43, 44, 45] and were partially included in previous discussions of precise MSSM neutral Higgs production cross sections [46]. Although for a pure CP-odd singlet component NNLO stop-induced contributions are the first non-vanishing contributions to the gluon fusion cross section, we leave an inclusion of these to future work. For completeness, we add that in the MSSM a numerical evaluation of NLO squark/quark/gluino contributions was also reported in Ref. [47, 48], whereas Refs. [49, 50, 51] presented analytic results for the pure squark induced NLO contributions. Electro-weak contributions to the gluon fusion production process mediated through light quarks [30, 31] can be adjusted from the SM to the MSSM [7] and similarly to the NMSSM and are known to capture the dominant fraction of electroweak contributions for a light SM-like Higgs with a mass below the top-quark mass, whereas they are generically small for larger Higgs masses.

For large values of , the ratio of the vacuum expectation values of the neutral components of the two Higgs doublets, the bottom-quark Yukawa coupling is enhanced, such that the bottom sector gets more important for gluon fusion, and the associated production with a pair of bottom-quarks is significantly enhanced. SusHi includes bottom-quark annihilation , which in case of non-tagged final state -quarks is a good theoretical approach, since it resums logarithms through the -parton distribution functions. The latter process is known as five-flavor scheme (5FS) up to NNLO QCD [52, 53] and can easily be reweighted from the SM to the MSSM/NMSSM by effective couplings [54, 55]. In the NMSSM the singlet does not couple to quarks at LO, however taking into account the singlet induced component into the resummation of higher-order sbottom effects is mandatory, since also the singlet to sbottom couplings are enhanced by .

The new release of SusHi thus provides gluon fusion cross sections at NLO QCD taking into account the third generation quarks and their superpartners, the squarks, for all the five neutral Higgs bosons of the NMSSM. The squark and squark/quark/gluino contributions are implemented in asymptotic expansions of heavy SUSY masses. Electro-weak corrections induced by light quarks through the couplings of the Higgs bosons to and bosons can be added consistently like in the MSSM. Similarly, the NNLO top-quark induced contributions are included. In addition, sbottom contributions can be resummed into an effective bottom-quark Yukawa coupling, also taking into account the additional singlet to sbottom couplings. The latter also applies to the calculated bottom-quark annihilation cross section at NNLO QCD. All features SusHi provides for the MSSM are available for the NMSSM as well, in particular distributions with respect to the (pseudo)rapidity and transverse momentum of the Higgs boson under consideration can be obtained. Left for future work is a link to MoRe-SusHi [56] to allow for the calculation of momentum resummed transverse momentum distributions.

We proceed as follows: We start with a discussion of the theory background in Section 2, where we elaborate on the NMSSM Higgs sector and the calculation of the gluon fusion cross section. Then we present the NLO virtual amplitude for gluon fusion as well as the calculation of bottom-quark annihilation including the resummation of sbottom-induced contributions to the bottom-quark Yukawa coupling in the NMSSM. Subsequently we comment on the implementation in SusHi in Section 3, before we investigate the phenomenological features of the singlet-like Higgs boson in the CP-even and CP-odd sector with regard to Higgs production in Section 4. We also include a short discussion of theoretical uncertainties. Finally, we conclude and present the Higgs-squark-squark couplings in Appendix A.

## 2 Theory background

In this section we discuss the Higgs sector of the CP-conserving -invariant NMSSM, before we proceed to the resummation of enhanced sbottom contributions in the bottom-quark Yukawa coupling. Subsequently we move to the discussion of the Higgs production cross section in gluon fusion, where we present the adapted formulas for the NLO SQCD virtual amplitude, and finally comment on the consequences of the additional singlet to bottom-quark annihilation.

### 2.1 The Higgs sector of the Cp-conserving Nmssm

Our notation of the Higgs sector of the CP-conserving -invariant NMSSM closely follows Ref. [57]. For NMSSM reviews we refer to Refs. [3, 4]. The superpotential can be written in the form

(1) |

where equals the superpotential of the MSSM without -term. denotes the additional SU singlet superfield compared to the MSSM with the two SU doublet superfields and . contracts the SU doublet components. Since the singlet is a neutral field, it induces one additional CP-even and one additional CP-odd neutral Higgs boson as well as one additional neutralino compared to the MSSM. The soft-breaking terms include the scalar components and of the superfields and are given by

(2) |

The soft-breaking mass can be derived from the minimization conditions of the tadpole equations (in addition to and like in the MSSM), whereas and are usually considered input parameters. can be alternatively replaced by the charged Higgs mass as input parameter. The neutral components of the Higgs fields are decomposed according to

(3) |

where and denote the vacuum expectation values (VEVs) and the fields with indices and are the CP-even and CP-odd fluctuations around them. An effective term is generated through the VEV of the singlet

(4) |

which will be further used within this article. We do not present the explicit form of the mass matrices here, but refer to Ref. [57]. We define the CP-even gauge eigenstate basis and the CP-odd one ). Whereas in the former case the mass eigenstates with are obtained through one rotation

(5) |

we perform a prerotation in the CP-odd sector to obtain the MSSM pseudoscalar and the Goldstone in the form . The prerotation is given by the ratio of vacuum expectation values , such that the mass eigenstates with are obtained by

(6) |

where is a -matrix, which however only consists of a -mixing block, whereas for and . For Higgs production the Goldstone boson does not need to be considered. In the following we make use of the notation “singlet-like Higgs boson”, which refers to the CP-even/odd Higgs boson with the dominant fraction of the singlet component in gauge eigenstates. For this purpose we define the singlet character for and for . In our discussion of cross sections we denote the Higgs boson by the letter , which can be replaced by any of the physical Higgs bosons or . For picking viable scenarios for phenomenological studies we refer to Ref. [58] for a recipe to obtain positive eigenvalues for the singlet-like CP-even and -odd Higgs by varying between a minimal and a maximal value.

Whereas the singlet component does not couple to quarks, -terms induce a coupling of the singlet-like Higgs to squarks, which is of relevance for Higgs production. We present the Higgs-squark-squark couplings to the third generation of squarks in Appendix A. We point out that the singlet component mixes with the Higgs doublets proportional to and also the couplings of the singlet component to squarks are proportional to . It is thus possible to mostly decouple the singlet component by lowering the value of the parameter . The couplings to quarks can be easily translated from the MSSM by the correct projection on the neutral doublet components , and the pseudoscalar and yield relative to the SM

(7) |

with in the CP-even and in the CP-odd Higgs sector. The relative strength enters the Yukawa couplings in the form with the vacuum expectation value .

### 2.2 Resummation of higher-order sbottom contributions

It is well-known in the MSSM that enhanced sbottom corrections to the bottom-quark Yukawa coupling can be treated in an effective Lagrangian approach [59, 60, 61, 62, 63, 64] to be resummed. For the case of the NMSSM just taking into account SQCD corrections the effective Lagrangian can be written in the form [65]

(8) | |||

(9) |

Ref. [65] additionally presents the inclusion of SUSY electroweak corrections proportional to the soft-breaking parameter . The inclusion of electroweak corrections into does not harm our subsequent discussion of SQCD corrections and can thus always be included in the bottom-quark Yukawa coupling entering gluon fusion and bottom-quark annihilation. Apart from a coupling of the bottom-quarks to the gauge eigenstate also an effective coupling to the singlet can be induced at loop level, the latter being proportional to instead of . The sbottom corrections can be absorbed into effective Yukawa couplings, which read [65]

(10) |

for the three CP-even Higgs field and

(11) |

for the two CP-odd Higgs fields .

### 2.3 Gluon fusion cross section

After our discussion of the CP-conserving NMSSM Higgs sector and the resummation of sbottom contributions in the bottom-quark Yukawa coupling, we present the gluon fusion production cross section for a Higgs boson , which can be written in the form [7]

(12) |

with and the hadronic centre-of-mass energy . The factor includes the LO partonic cross section. encodes NLO terms of singular nature in the limit with the partonic centre-of-mass energy . The gluon-gluon luminosity is given by the integral

(13) |

The contributions , , and are the regular terms in the limit in the partonic cross section and arise from , and scattering, respectively. The LO contribution is obtained by the formulas presented in Ref. [7] using the NMSSM couplings of the Higgs bosons to quarks and squarks. Similarly the contributions are obtained from the MSSM by a proper replacement of the involved Higgs boson to quark and squark couplings. The factor can be decomposed in the form

(14) |

with and as well as the factorization and renormalization scales, and respectively. is the LO (one-loop) virtual amplitude in the limit of large stop and sbottom masses. is the NLO (two-loop) virtual amplitude and equals the form factors for the CP-even Higgs bosons and for the CP-odd Higgs bosons, which are presented in the following Section 2.4 to account for NLO virtual contributions from quarks and squarks in an appropriate way. In the MSSM limit they correspond to the form factors of Refs. [36, 37, 38] except from a constant factor of . Contrary to the case of the MSSM we do not employ evalcsusy [40, 41] to obtain the NLO amplitude in the limit of heavy top-quark and stop masses for the light Higgs, but use the expanded form factors presented in the following sections instead. Accordingly our implementation does not (yet) include approximate NNLO stop contributions as presented in Ref. [46] for the MSSM. The NNLO top-quark contributions in the heavy top-quark effective theory making use of Refs. [15, 66] are included according to Eq. (29) of Ref. [7].

Lastly we comment on the inclusion of the electroweak corrections to the gluon fusion production cross section. Similarly to the MSSM the full SM NLO electroweak (EW) corrections [29] can be added to the top-quark induced result only, assuming complete factorization of EW and QCD effects [67]. We recommend the latter procedure only for a SM-like Higgs boson. Contrary the inclusion of electroweak corrections due to light quarks [30, 31], where the Higgs boson couples to either the or boson, can be adjusted to the MSSM and accordingly the NMSSM in an appropriate way [68]. For this purpose the generalized couplings

(15) |

of the -th CP-even NMSSM Higgs boson to the heavy gauge boson need to be inserted in the formulas of Ref. [7]. The missing projection on the singlet component reflects the fact that the singlet does not couple to gauge bosons. The CP-odd Higgs bosons do not couple to gauge bosons either, such that electroweak corrections due to light quarks are absent.

### 2.4 Nlo virtual amplitude for gluon fusion

Regarding the implementation of two loop contributions to gluon fusion, we closely follow Refs. [36, 37, 38] for the MSSM, which can be translated to the NMSSM. Their calculation at NLO is based on an asymptotic expansion in the masses of the supersymmetric particles. We can project the form factors onto the ones in gauge eigenstates according to

(16) | ||||

(17) |

The individual contributions in gauge eigenstates are presented in Section 2.4.1 for the CP-even and in Section 2.4.2 for the CP-odd Higgs bosons. We included the constant factor between Refs. [36, 37, 38] and our work in the above equations.

#### 2.4.1 CP-even Higgs bosons

In this subsection we present the form factors for the CP-even Higgs bosons
in gauge eigenstates^{1}^{1}1In the CP-even sector we adapt the MSSM results of Refs. [36, 38]
to the NMSSM by isolating the terms proportional to the -squark-squark couplings and replacing
them by the -squark-squark couplings for the form factor .
Similarly we proceed in the CP-odd sector starting from the form factors of Ref. [37]
taking into account the prerotation of the CP-odd Higgs mixing matrix.

(18) |

which includes the effective parameter defined in Eq. (4). All functions in , and can be directly taken over from Refs. [36, 38], keeping in mind the different convention in the sign of the parameter. For on-shell (OS) parameters (see Refs. [36, 38]) and thus for our implementation the contribution is shifted according to Section 3.3 of Ref. [38] and according to Ref. [36]. The shift also applies to and entering the singlet contribution , since the differences in the prefactors being , or are not renormalized when taking into account SQCD contributions and therefore do not contribute to the described OS shifts.

It remains to discuss the inclusion of resummed sbottom contributions into the bottom-quark Yukawa coupling within the virtual corrections to gluon fusion, where care has to be taken to avoid a double-counting of NLO SQCD contributions. The naive resummation is incorporated in the same way as in case of the MSSM [36, 46]. The resummation as presented in Section 2.2 instead needs the subtraction of the enhanced contributions to multiplied with the corresponding coupling correction, in detail for the three CP-even Higgs bosons

(19) |

with the factor being

(20) |

All occurrences of the bottom-quark Yukawa coupling in the two-loop amplitude are multiplied with the factor using Eq. (10), such that the shift reported in Eq. (19) avoids double-counting of the purely SQCD induced contributions at the two-loop level. Employing the expansion in heavy SUSY masses the NLO virtual contributions to neutral CP-even Higgs production in the NMSSM are now fully presented.

#### 2.4.2 CP-odd Higgs bosons

We now turn to the case of the two CP-odd Higgs bosons, where we present the form
factor in the basis after a prerotation from gauge eigenstates^{1}^{1}footnotemark: 1.
At LO only diagrams involving quarks coupling to the pseudoscalar exist, such that
the form factor at LO only consists of the part , whereas equals zero.
At NLO however couplings of and to
squarks for induce contributions to Higgs production.
The two-loop form factor presented in Ref. [37] for the
MSSM can therefore be translated to

(21) |

Whereas the individual contributions to can be taken from Ref. [37], we present the contributions to separately:

(22) | ||||

(23) |

with and . The functions and can be found in Ref. [37]. The functions and are given by:

(24) | ||||

(25) |

In the bottom sector the relevant function yields:

(26) |

The shifts of individual contributions in case of OS parameters can be taken over from the MSSM case. The inclusion of resummed sbottom contributions to the bottom-quark Yukawa coupling needs the following shift in the two-loop form factor for the CP-odd Higgs bosons

(27) |

using

(28) |

Again we point out that our sign convention with respect to is opposite to Ref. [37] and all occurrences of the bottom-quark Yukawa coupling in the two loop amplitude are multiplied with the factor using Eq. (11).

### 2.5 Bottom-quark annihilation cross section in the 5FS

The generalization of the calculation of bottom-quark annihilation cross sections in the five-flavor scheme (5FS) from the MSSM to the NMSSM case is straightforward by using the appropriate couplings of Higgs bosons to bottom-quarks. For this purpose the resummation of sbottom contributions as described in Section 2.2 is taken into account. For the specific case of the singlet-like Higgs boson we point out that in case the coupling to the bottom-quark vanishes (due to cancellations in the mixing with the Higgs doublets) a priori the coupling to sbottom squarks can still be present. This is not taken into account by the resummation procedure.

## 3 Implementation in SusHi

In the current implementation of neutral Higgs production in the real NMSSM within the code SusHi the Higgs mixing matrices as well as the Higgs masses have to be provided as input in SUSY Les Houches Accord (SLHA) form [69, 70] and can be obtained by spectrum generators for the NMSSM. Common codes are NMSSMTools [71, 72, 73, 74], NMSSMCALC [75, 76, 57, 65, 77], SOFTSUSY [78, 79], SPheno+Sarah [80, 81, 82] and FlexibleSUSY+Sarah [80, 83].

Special attention needs to be paid to the renormalization of the stop and sbottom sector, which in the ideal form should be identical in the calculation of Higgs masses and mixing and the calculation of Higgs production cross sections. For the time being, SusHi either relies on the internal calculation of on-shell stop and sbottom sectors as described in the manual [7] or on the specification of the on-shell masses and and mixing angles in the input file. For both cases input files can be found in the folder /example within the SusHi tarball. The user is asked to check the meaning of output parameters of spectrum generators, i.e. the chosen renormalization scheme. If the user specifies the on-shell squark masses and mixing angles together with the on-shell soft-breaking parameters and by hand, she/he should make sure that in the stop sector as well as the on-shell top-quark mass , the on-shell stop masses and and the mixing angle fit the formula

(29) |

In the sbottom sector on-shell and tree-level masses on the other hand differ by a shift in the -element, see in Ref. [7]. Moreover we employ the scheme which works with a dependent bottom-quark mass , whereas is defined to be on-shell, see e.g. Refs. [84, 85, 86]. To allow for maximal flexibility the specification of on-shell squark masses and mixing angles is now also possible in case of the MSSM. The Block RENORMSBOT is not of relevance in such input files, since is chosen as dependent parameter, whereas the squark mixing angle and the soft-breaking parameter are understood as renormalized on-shell.

Two options for the pseudoscalar Higgs mixing matrix are accepted as input by SusHi, namely the full Higgs mixing matrix, which corresponds to the multiplication in the above notation, but instead also the rotation matrix can be used as input. Following SLHA2 [70] the full matrix is provided in Block NMAMIX and asks for entries with and . The matrix can be specified in Block NMAMIXR, which only asks for entries with . We point out that in contrast to other codes the Goldstone boson remains the first mass eigenstate, such that Block NMAMIXR does not ask for entries with or . The elements of the CP-even Higgs boson mixing matrix are specified in Block NMHMIX [70]. The Higgs masses need to be given in Block MASS using entries and for the CP-even Higgs bosons and , for the CP-odd Higgs bosons.

The block Block EXTPAR still contains the gluino mass as well as the soft-breaking parameters for the third generation squark sector. Entry for the parameter is however replaced by entry , where the effective value of needs to be specified. Moreover entry asks for the choice of . SusHi extracts the VEV from and . Since the Higgs sectors including their mixing are provided, there is no need to provide the parameters , , (or ) in the SusHi input, since they do not enter the couplings relevant for Higgs production. The Block SUSHI entry specifies the Higgs boson, for which cross sections are requested. The CP-even Higgs bosons are numbered and , the CP-odd Higgs bosons and . Similarly the options and also work in the 2-Higgs-Doublet Model (2HDM) and the MSSM and and in the SM. A CP-odd Higgs boson in the SM is obtained from the 2HDM case with . We note that SusHi is still compatible with input files with (light Higgs), (pseudoscalar) and (heavy Higgs) as options for entry . Output files however stick to the new convention.

For the time being we emphasize that SusHi is not strictly suitable for very low values of Higgs masses GeV, where quark threshold effects start to become relevant and also electroweak corrections are not implemented. This statement mostly applies to studies of a very light CP-odd Higgs boson, which is poorly constrained by LEP experiments in contrast to a light CP-even Higgs boson [87].

## 4 Phenomenological study

In this section we elaborate on the phenomenological consequences of the additional SU singlet in the NMSSM with respect to the MSSM for neutral Higgs production. Neglecting the squark induced contributions to gluon fusion, the only consequence of the additional singlet component is another admixture of the three CP-even/two CP-odd Higgs bosons. However, no generically new contributions to Higgs boson production arise. This differs when taking into account squark induced contributions to gluon fusion due to the additional singlet to squark couplings. In particular for the CP-odd Higgs bosons squark contributions are only induced at the two-loop level due to the non-diagonal structure of the CP-odd Higgs bosons to squark couplings. Subsequently we work with two scenarios, start with their definition, present the Higgs boson masses and admixtures and then discuss the behavior of cross sections, including the squark and electroweak corrections to the gluon fusion cross section. Our studies are performed for a proton-proton collider with a centre-of-mass (cms) energy of TeV, as planned for the second run of the LHC. Lastly we add a short discussion of renormalization and factorization scale uncertainties as well as PDF uncertainties for one of the two scenarios.

### 4.1 Scenarios and

To present the most relevant features of the NMSSM for what concerns
neutral Higgs production we pick two scenarios. The first scenario is in the vicinity
of the natural NMSSM [5] with a rather large value of .
Other input parameters are GeV, GeV, TeV,
, GeV
and GeV. is determined from the charged Higgs
mass GeV.
The size of ensures a large mixing of the singlet component
with the and doublets.
All soft-breaking masses are set to TeV except
for the soft-breaking masses of the third generation squark sector, which
are fixed to GeV. The soft-breaking couplings are set to TeV.
The on-shell stop masses are then given by GeV
and GeV, whereas the sbottom masses are GeV
and GeV.
We vary between and
and thus vary the mass of the singlet-like Higgs component in particular
in the CP-even Higgs sector. We note that for illustrative reasons
the perturbativity limit approximately given by is not
always fulfilled in our study.
We work out the characteristics
for the singlet-like component in the following discussion.
The relevant input for SusHi is obtained
with NMSSMCALC 1.03, which incorporates the leading two-loop
corrections to the Higgs boson masses
calculated in the gaugeless limit with vanishing external momentum [77].
We request NMSSMCALC to work with an on-shell renormalized stop sector
and add local modifications to the NMSSMCALC input routines to read in on-shell
parameters rather than renormalized parameters^{2}^{2}2We thank Kathrin Walz for
instructions on how to modify the NMSSMCALC input routines..
These modifications guarantee identical on-shell stop masses
in NMSSMCALC and SusHi. The renormalization of the sbottom
sector on the other hand is performed SusHi-internally.

We also choose a second scenario , in which we vary to decouple the singlet-like Higgs from the Higgs doublets. The detailed choice of parameters is GeV, GeV, TeV, , TeV, , GeV, GeV and GeV. In this scenario we set the soft-breaking masses to TeV. The on-shell stop and sbottom masses are given by GeV, GeV, GeV and GeV. We vary between and . For small values of corresponds to the SM-like Higgs boson with mass GeV. The lower bound at is to avoid tiny cross sections for a heavy singlet-like Higgs boson and to keep its mass below the SUSY masses thresholds to justify the NLO SQCD expansion employed for the gluon fusion cross section calculation.

Both our scenarios come along with rather light third generation squark masses at the low TeV scale. Contrary to the Higgs mass calculations the squark contributions completely decouple from Higgs production for heavy SUSY spectra. Our scenarios are chosen to flash the phenomenology of an additional singlet-like Higgs boson and thus do not always include a SM-like Higgs boson with mass GeV and are partially under tension from LEP searches [87] (for low CP-even Higgs masses below GeV) or LHC searches [88, 89, 90, 91, 92, 93, 94, 95, 96, 97, 98, 99, 100, 101, 102].

We add for both scenarios the relevant SM input, which includes the renormalized bottom-quark mass GeV, which is translated into a bottom-quark pole mass of GeV. In SusHi we choose the renormalization scheme, where the bottom-quark pole mass enters all occurrences of heavy bottom-quark masses in the loops and the bottom-quark Yukawa coupling for the gluon fusion cross section. Bottom-quark annihilation is based on the running renormalized bottom-quark Yukawa coupling. As pointed out in Ref. [46] the gluon densities are hardly dependent on the bottom-quark pole mass fit value of the PDF fitting groups, emphasizing that there is no need to adjust the bottom-quark pole mass to the PDF fit value for the calculation of the gluon fusion cross section. The top-quark pole mass equals GeV. The strong coupling constant is set to for the calculation of running masses, and is obtained from the corresponding PDF set for the cross section calculation. We choose MSTW2008 [103] at the appropriate order in perturbation theory. Our central scale choices for gluon fusion are for both renormalization and factorization scale, and respectively, and and for bottom-quark annihilation.

### 4.2 Higgs boson masses and singlet admixtures

(a) | (b) |

(c) | (d) |

Subsequently we start with a discussion of the singlet admixture and the masses of the three CP-even and the two CP-odd Higgs bosons, which we obtain through a link to NMSSMCALC 1.03 as explained beforehand. For scenario the singlet component as a function of for the three CP-even Higgs bosons is shown in Fig. 1 (a). Clearly, for low values of the lightest Higgs is mainly singlet-like, whereas with increasing the dominant singlet fraction moves from to and for large values of to . The sum of all singlet components yields . The masses of the CP-even Higgs bosons can be found in Fig. 1 (b). With increasing the mass term of the singlet component in gauge eigenstates is increasing proportional to , such that the singlet-like Higgs boson can be identified with the Higgs boson linearly increasing in mass. Close to shows the most dominant singlet fraction, which will later be visible in the gluon fusion cross section. Scenario includes for a SM-like Higgs boson with a mass of GeV. For very small values of the decay opens and leaves a characteristic signature for the SM-like Higgs boson . Note that a light singlet-like Higgs boson lifts the mass of the SM-like CP-even Higgs through singlet-doublet mixing, which for our example equals GeV for . The region of small and a light CP-even singlet-like Higgs boson is largely constrained by the LEP experiments [87].

Fig. 1 (c) and (d) show the behavior of the singlet admixture and the masses for the two CP-odd Higgs bosons in scenario as a function of . We point again to the region in the vicinity of , where the light CP-odd Higgs boson is a pure singlet-like CP-odd Higgs boson contrary to the CP-even Higgs boson , for which and components remain. The coupling of to quarks vanishes, but the coupling to squarks is still present due to the relatively large value of , which will be apparent when calculating the gluon fusion cross section.

(a) | (b) |

(c) | (d) |

For scenario Fig. 2 shows correspondingly the singlet character and masses for the CP-even and CP-odd Higgs bosons. Due to the fixed value of the singlet-like Higgs boson increases in mass (proportional to ) with decreasing and thus for small as well as clearly decouple from the other Higgs bosons. We will later use this setup to show the decoupling behavior of the cross sections. Below both and have a singlet character, which exceeds .

### 4.3 Scenario : Inclusive cross sections for TeV

In this subsection we investigate the gluon fusion and bottom-quark annihilation cross sections for scenario for TeV for a proton-proton collider. The subsequent statements are however hardly dependent on the cms energy and thus hold for the TeV LHC runs as well as for more energetic runs. Fig. 3 shows the cross sections for the three CP-even Higgs bosons. Naturally the cross sections are strongly dependent on the Higgs mass, which are in turn a function of . Thus, the cross section for the second CP-even Higgs bosons tends to decrease with increasing . Crucial is the singlet admixture of the Higgs boson under consideration. The larger the singlet component , the smaller the coupling to quarks becomes and thus the more sensitive is the cross section to squark and electroweak contributions. For we observe a cancellation of quark contributions through the admixtures with the SU doublets around , where in turn due to the generally small cross section squark but also electroweak corrections to the gluon fusion cross section are of large relevance, see Fig. 3 (c) and (d). For small values of the decay opens in addition to the large gluon fusion cross section for the singlet-like CP-even Higgs boson . The region is therefore constrained by LEP experiments [87]. Much smoother is the behavior for the bottom-quark annihilation cross section, where the direct coupling to bottom-quarks is related to the non-singlet character of the Higgs under consideration. In an interval around bottom-quark annihilation even exceeds the gluon fusion cross section for despite the small value of .

(a) | (b) |

(c) | (d) |

We show the effect of squark and electroweak contributions to gluon fusion for the three CP-even Higgs bosons in Fig. 3 (c) and (d). in Fig. 3 (c) includes stop- and sbottom-quark induced contributions at NLO SQCD on top of the quark induced contributions without electroweak contributions and compares to the pure quark induced cross section without electroweak contributions. All cross sections include NLO QCD quark contributions and the NNLO QCD top-quark induced contributions in the heavy top-quark effective theory. Fig. 3 (d) accordingly shows the effect of electroweak contributions induced by light quarks following Eq. (15) in combination with Ref. [46] in comparison to the quark and squark induced cross section . Note that in all our figures corresponds to . As expected for the region with small quark contributions induced by the admixture with the and components is in particular sensitive to squark corrections. For the other Higgs bosons the squarks corrections in this scenario are incidentally all of the order of %) and mostly independent of . We note that the squark corrections are mainly induced by stop contributions, whereas sbottom-induced contributions only account for a small fraction. Interestingly, the squark contributions show an interference-like structure with a maximum and minimum around , whereas the relative electroweak corrections are always positive. This can be understood from a sign change in the real part of the quark induced LO and NLO amplitude for at , which is of relevance for the squark contributions, whereas the imaginary part, more relevant for the electroweak contributions, does not change its sign. The size of the electroweak corrections for follows from a suppression of the couplings of the second lightest Higgs to quarks in contrast to the couplings to gauge bosons. Obtaining a pure singlet-like Higgs boson in the CP-even Higgs sector, which neither couples to quarks and gauge bosons, rarely happens due to the mixing between both and as well as and for large values of . For the SM-like Higgs boson with a mass below the top-quark mass the electroweak corrections by light quarks are typically of the order of %) and cover most of the SM-electroweak correction factor. On the other hand, for Higgs masses above the thresholds or the electroweak corrections by light quarks are small. The structure visible for in Fig. 3 (c) for is induced by the thresholds and , which the Higgs mass crosses between and . We leave the distortion of distributions, in particular transverse momentum distributions, for such a scenario to future studies.

Similarly we depict the gluon fusion and bottom-quark annihilation cross sections for the two CP-odd Higgs bosons in Fig. 4 (a) and (c). The pure singlet-like Higgs boson at is clearly apparent, since both cross sections vanish. The corrections through squark contributions as shown in Fig. 4 (b) are very large around , since squark contributions are not suppressed through Higgs mixing, although they only appear at NLO SQCD. Electro-weak corrections induced through light quarks are absent for the CP-odd Higgs bosons. We note that in the range , where the LO QCD gluon fusion cross section for the light CP-odd Higgs boson are tiny, pb, the prediction for with squark induced NLO SQCD contributions for is unreliable, since SusHi calculates NLO QCD contributions through the multiplication of one-loop and two-loop contributions, where the latter tend to be significantly larger than the former and can thus even induce negative cross sections. However, in these regions the tiny cross sections are not of relevance for current searches. The cross section and the relative correction to the vanishing only quark induced cross sections of more than % need to be taken with care for the CP-odd Higgs bosons. The fact that for a pure singlet-like CP-odd Higgs boson the gluon fusion cross section at NLO SQCD completely vanishes due to the absence of a LO contribution motivates to take into account NNLO SQCD stop contributions as it was done for the light CP-even Higgs boson in Ref. [46]. A first estimate yields tiny, positive cross sections, but we leave an inclusion in SusHi to future work. The CP-even Higgs bosons in contrast have a LO squark induced contribution, which leaves mostly well-behaved. Only in rare cases, where LO squark and quark contributions cancel, similar difficulties can arise.

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### 4.4 Scenario : Inclusive cross sections for TeV

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