Precision Probes of a Leptophobic Z^{\prime} Boson

# Precision Probes of a Leptophobic Z′ Boson

Matthew R. Buckley and Michael J. Ramsey-Musolf Center for Particle Astrophysics, Fermi National Accelerator Laboratory, Batavia, IL 60510, USA Department of Physics, University of Wisconsin, Madison, WI 53706, USA Kellogg Radiation Laboratory, California Institute of Technology, Pasadena, CA 91125, USA
July 12, 2019
###### Abstract

Extensions of the Standard Model that contain leptophobic gauge bosons are theoretically interesting but difficult to probe directly in high-energy hadron colliders. However, precision measurements of Standard Model neutral current processes can provide powerful indirect tests. We demonstrate that parity-violating deep inelastic scattering of polarized electrons off of deuterium offer a unique probe leptophobic bosons with axial quark couplings and masses above 100 GeV. In addition to covering a wide range of previously uncharted parameter space, planned measurements of the deep inelastic parity-violating asymmetry would be capable of testing leptophobic scenarios proposed to explain the CDF plus di-jet anomaly.

preprint: FERMILAB-PUB-12-049-Apreprint: NPAC-12-03

The addition of a new abelian gauge group is one of the simplest extensions to the Standard Model (SM) that can be considered. In principle, a completely generic and its associated gauge boson, the , could have arbitrary generation-dependent couplings to the known particles, with the resulting triangle anomalies cancelled by the addition of new heavy chiral fermions. The resulting embarrassment of (theoretical) riches arising from this freedom of choice calls for the addition of a guiding symmetry principle as to impose some amount of order. Widely considered gauge groups (see, for example the reviews Refs. Nakamura:2010zzi (); Langacker:2008yv () and references therein) include gauged (the unique choice that is anomaly free with the Standard Model fermion content), with a free parameter, Grand Unified Theory (GUT)-derived models, and leptophilic bosons. The latter have held particular interest recently in the context of explaining the PAMELA Adriani:2008zr () and Fermi Abdo:2009zk () anomalies in terms of dark matter ArkaniHamed:2008qn (); Essig:2009nc ().

The majority of the models that have been studied contain sizable couplings to leptons – an important feature as the dominant experimental constraints come from processes involving leptons (for a recent global analysis, see Ref. Erler:2011iw ()). For example, a sequential , whose couplings to SM fermions are proportional to those of the , is ruled out for below  TeV. Similar constraints hold for other scenarios with leptonic couplings Nakamura:2010zzi (). Intriguingly, bosons that couple exclusively (or at least predominantly) to quarks are not as strongly limited by collider experiments, due to the large QCD backgrounds. The most obvious channel for a leptophobic search at hadronic machines, , is stymied at low mass by the prohibitive dijet background rate. Currently, the tightest bound in this channel for a below  GeV with electroweak-scale couplings comes from the UA2 experiment Alitti:1993pn () (see also Refs. Buckley:2011vc (); Yu:2011cw ()).

In the last year, the CDF collaboration reported an excess of events in the channel, seen as a Gaussian peak in the distribution at  GeV Aaltonen:2011mk (). This anomaly, initially reported at in 4.3 fb, growing to in 7.3 fb CDF2 (), can be interpreted as a new coupling to quarks with a mass of  GeV and a charge times gauge coupling of Buckley:2011vc (); Yu:2011cw (); Cheung:2011zt (). Particular theoretical realizations of such leptophobic models have since been considered; for example, separately gauged and Buckley:2011vs (), or a GUT with hypercharge- mixing Buckley:2011mm (). A DØ search does not see a similar excess Abazov:2011af (), and disagreement between the two experiments remains. The situation is unlikely to be fully resolved until ATLAS and CMS weigh in with  fb of data Eichten:2011xd (); Buckley:2011hi ().

Regardless of the final resolution of this particular anomaly, it is clear that leptophobic gauge groups are both theoretically interesting and not well constrained by existing searches. In this paper, we propose a new precision probe of leptophobic bosons using parity-violating deep inelastic scattering (PV-DIS) of electrons off of deuterium. Historically, PV-DIS played a key role in singling-out the Glashow-Weinberg-Salaam prediction for the neutral weak interaction from among alternative possibilities. From a theoretical perspective, it has often been considered as a potentially powerful indirect probe of possible physics beyond the Standard Model (see, e.g., RamseyMusolf:2006vr (); Erler:2004cx (); Robinett:1981yz () and references therein). In the present era, a measurement of the PV asymmetry has recently been completed with the GeV beam at Jefferson Lab (JLab) Subedi:2011zz (), while more precise measurements are planned for the JLab 12 GeV program SOLID (), and discussed as a possibility for a future Electron Ion Collider (EIC) Boer:2011fh ().

As we will show, the future PV-DIS asymmetry measurements would be sensitive to axial couplings to quarks of a with mass and couplings required to explain the CDF anomaly. Furthermore, these measurements would be competitive with the current leading experimental bounds. In what follows, we use the leptophobic model of Ref. Buckley:2011mm () as a benchmark scenario, but provide a more general framework for assessing the leptophobic scenario.

The effect of new physics on parity violation in deep inelastic scattering is parameterized by four couplings in the effective Lagrangian:

 LPV=GF√2∑q[C1q(¯eγμγ5e)(¯qγμq)+C2q(¯eγμe)(¯qγμγ5q)]. (1)

Here, the sum is over the valence quarks (). In the SM, these couplings are (see, e.g., Ref.  RamseyMusolf:2006vr ())

 C1q = 2^ρNCIe3(Iq3−2Qq^κsin2^θW)−12^λq1 (2) C2q = 2^ρNCIq3(Ie3−2Qe^κsin2^θW)−12^λq2   , (3)

where is the third component of weak isospin for fermion , is the electromagnetic charge, and angle is the weak mixing in the scheme. The quantities , , and encode the effects of electroweak radiative corrections and at tree-level take on the values 1, 1, and 0, respectively. Theoretically, the and are predicted to better than one percent precision. Experimentally, the nuclear weak charge has been determined at the level by measurement of PV transitions in cesium Wood:1997zq (); Porsev:2009pr (), while the proton weak charge will be determined to precision with PV elastic scattering at JLab by the Q-Weak Collaboration QWeak (). Note that at tree level , so that a 4% determination of this quantity is roughly comparable to a 0.5% determination of the cesium weak charge. For a summary of present and prospective constraints on the see Ref. Young:2007zs ().

In contrast, the present experimental bounds on the are considerably weaker, a situation that would be remedied by the PV-DIS studies. Experimentally, the projected precision of the SOLID experiment would yield a determination of with an uncertainty SOLID (). An EIC measurement could lead to a factor of two-to-three smaller uncertainty, provided an ultra-high luminosity version is ultimately constructed, with an integrated luminosity of 0.5 to 1 attobarn KK ().

The PV asymmetry is sensitive to both the and :

 AeDPV = −GμQ22√2πα910[~a1+~a21−(1−y)21+(1−y)2], (4)

where is the Fermi constant as determined from the muon lifetime, the parameter is the square of the four momentum transfer, and the are given by

 ~a1 = −23(2C1u−C1d)[1+R1], ~a2 = −23(2C2u−C2d)[1+R2].

Here the denote various hadronic corrections, including those associated with higher twist contributions to the deep inelastic structure functions and charge symmetry violation (CSV) in the parton distribution functions (for recent discussions, see Refs. Mantry:2010ki (); Hobbs:2008mm ()). Through an appropriate program of measurements at different kinematics ( and Bjorken-), it is in principle possible to disentangle these hadronic contributions from the - and -dependent terms.

In general, new physics could become apparent in both and . Given the sensitivity of the cesium atomic PV and Q-Weak experiments to the , it is relevant to ask what complementary information a determination of the coefficients from might provide. In this context, the leptophobic scenario is particularly interesting, as it will not affect the at an appreciable level but could lead to a sizeable shift in the as we show below.

Since (by assumption) the does not couple to the electrons, its dominant contribution to the operator arises at one-loop level through mixing tensor as shown in Fig. 1. The leptophobic couples only to quarks in the loop, in contrast to analogous mixing in the SM that also includes lepton loops. The corresponding effect does not enter the operator proportional to as the photon has no tree-level axial coupling to the lepton and since the vertex vanishes. In principle, the analogous process involving mixing would lead to shifts in both and . However, the mixing angle is constrained to be Erler:2009ut (), rendering the effect too small to be observable in the next generation of experiments.111The specific mechanism for ensuring sufficiently small mixing requires a detailed discussion of the scalar sector of the extension, a topic that goes beyond the scope of the present work. See e.g. Refs. Hewett:1985ss (); Hewett:1986bk (); Cvetic:1997ky (); Amini:2002jp () and references therein for treatments within the context of supersymmetric models.

In what follows, we illustrate the prospective sensitivity of the PV-DIS asymmetry to exchange. We observe that the expected shift is enhanced relative to the naïve expectation of by two effects: the sum over quark colors and the presence of large logarithms that arise at the relatively low- of the PV-DIS experiments. In addition, the SM predictions for the are suppressed, as the tree-level values are proportional to , leading to an additional transparency to a mixing contribution that does not carry this suppression factor.

We first review the computation of the tree-level contribution to coefficient that arises from scattering via a SM -boson. We define the axial and vector couplings to the and gauge bosons via the Lagrangian

 L = ∑fgcosθW¯fγμ[QV,f+QA,fγ5]fZμ (5) +g′¯fγμ[Q′V,f+Q′A,fγ5]fZ′μ, QV,f = 12(I3,f−2Qfsin2θW), (6) QA,f = −12I3,f   , (7)

where we have dropped the hat notation from Eqs. (2) and (3) for simplicity. Here, the coupling is the gauge coupling, while the new gauge coupling and charges and are model dependent.

In terms of the vector and axial charges to electrons ( and ) and quarks ( and ), the scattering matrix element is

 iMtree = ig2cos2θW1q2−M2Z× [¯eγμ(QV,e+QA,eγ5)e][¯qγμ(QV,q+QA,qγ5)q].

Taking the limit, comparing to the effective Lagrangian in Eq. (1), and using , leads to the tree-level :

 C2q = −8QV,eQA,q (9) = 2I3,q(I3,e−2Qesin2θW), C2u = −12(1−4sin2θW)=−0.0372, (10) C2d = +12(1−4sin2θW)=+0.0372. (11)

Including the electroweak radiative corrections scheme indicated in Eq. (2), one obtains ,  Nakamura:2010zzi (), yielding . Thus, the projected sensitivity on of the SOLID experiment is approximately of the SM value.

A substantial contribution to the SM corrections arises from mixing that enters the quantity in Eq. (2). This quantity depends on both and the t’Hooft (renormalization) scale , while the product is -independent. Choosing , as is appropriate when comparing to -pole precision observables (), we encounter large logarithms in the theoretical predictions for the low- asymmetries of interest here. In this case, renormalization group (RG) improved predictions can be obtained by choosing and exploiting the RG evolution of as discussed in Ref. Erler:2004in (). Doing so resums the large logarithms by moving them from into .

Next, we consider the contribution. For purposes of illustrating the magnitude of this effect, we will defer a full RG-improved analysis to future work, concentrating instead on the contribution to given its conceptual simplicity. Following the approach of Ref. Marciano:1983ss (), we define for general gauge bosons and

 ΠμνVV′(q2) = i∫d4xe−iq⋅x⟨0|^TJμV(x)JνV′(0)|0⟩∣∣∣T (12) ΠμνVV′(q2) = (qμqν−q2gμν)ΠVV′(q2), (13)

where the is the time-ordering operator, () is the current that couples to vector boson (), and the subscript “” denotes the transverse component. With this normalization, the matrix element for scattering via the loop diagram shown in Fig. 1 is given by

 iM=ieg′ΠγZ′(q2)q2−M2Z′[¯eγμe][¯qγμ(Q′V,q+Q′A,qγ5)q]. (14)

Again taking the low limit and factoring out in order to compare with Eq. (1), we find

 iMPVγZ′ = iGμ√2[8cos2θWsinθW(g′g)(MZMZ′)2Q′A,q] (15) × ΠγZ′(q2)[¯eγμe][¯qγμγ5q].

We now turn to calculating . For heavy quarks (, , ), the one-loop perturbative calculation yields a reliable result Marciano:1983ss ():

 [ΠγZ′(0)]c,b,t = −Nceg′2π2∑qQqQ′V,qF(m2q,Q2), (16) F(m2q,Q2) = ∫10dx x(1−x)ln[m2q+x(1−x)Q2M2Z],

where is the number of quark colors.

However, as the light quarks (, , and ) have masses at or below the QCD scale, we must take non-perturbative effects into account. Following Ref. Marciano:1983ss (), we proceed by splitting the light quark contribution to the tensor into isovector and isoscalar contributions, leading to :

 ΠγZ′(q2) = eg′[(Q′V,u−Q′V,d)ΠI=1+ 13(Q′V,u+Q′V,d)ΠI=0+∑q=s,c,b,tQqQ′V,qΠq] .

Note that we have included the top quark in the sum, in contrast to the conventional treatment of Marciano:1990dp (); Fanchiotti:1992tu (). In the latter instance, one absorbs effects of order in the definition of , a quantity that one extracts from precision -pole observables. In the case, however, the top contribution to induces a non-vanishing vector coupling that does not exist at tree-level. Consequently, it is not possible to absorb these loop effects in the definition of renormalized vector couplings to leptons.

For the three light quarks, data from scattering to hadrons can be used to estimate the functions at :

 ΠI=0(0)=ΠI=1(0)=0.178, (18) Πs(0)=0.292. (19)

The and quark contributions can be reliably calculated from Eq. (16). If we replace with and with the Standard Model vector charges in Eq. (Precision Probes of a Leptophobic Boson) we reproduce the standard one-loop quark contribution , which contributes to both and the running of Marciano:1983ss (); Marciano:1982mm (); Czarnecki:1995fw ().

Combining Eqs. (15)-(19), we see that, in the limit, the shift in due to a gauge boson is

 ΔC2q = 32παcos2θW(g′g)2(MZMZ′)2Q′A,q× [23(2Q′V,u−Q′V,d)(0.178)−13Q′V,s(0.292)+ 23Q′V,c(0.210)−13Q′V,b(0.150)−23Q′V,t(0.032)].

To investigate the experimental sensitivity to this contribution, we select as a benchmark model the leptophobic GUT scenario outlined in Ref. Barger:1996kr () (and applied to the recent CDF excess Aaltonen:2011mk (); CDF2 () in Ref. Buckley:2011mm ()). In this model, the charges of the Standard Model particles are well defined. For the up- and down-type quarks they are:

 Q′V,u=16, Q′A,u=−12, (21) Q′V,d=−13, Q′A,d=0. (22)

With this normalization of the charges, in order to explain the overall cross section of the CDF excess, the gauge coupling constant must be . The dijet excess is observed at  GeV, and so for this work we take  GeV. Using these nominal values, in our leptophobic benchmark, we find at

 (ΔC2u)E6 = −0.0155(150 GeVMZ′)2(g′0.6)2, (23) (ΔC2d)E6 = 0. (24)

This corresponds to a correction to the SM value for . The lack of correction to is a model-dependent feature of the leptophobic , and is not generically expected of a new with axial charges. The future PV-DIS experiments will be carried out at non-zero , so one must evolve the result in Eq. (Precision Probes of a Leptophobic Boson) to the appropriate kinematic regime. To that end, we follow Ref. WJMSLAC (), and use the perturbative result in Eq. (16) with “effective” light quark masses: MeV, MeV, and MeV – choices that yield a good fit to the dispersive result. For the kinematics of the SOLID experiment, this parameterization leads to a reduction in the magnitude of by () at the lower (upper) end of the kinematic range.

The correction to from this scenario could conceivably be probed at the () level by SOLID (EIC). Looking past our benchmark model, such PV-DIS experiments could therefore serve as key tests for interpretation of the CDF dijet excess as resulting from a with axial couplings to quarks, though it must be noted that models with purely vectorial couplings (such as gauged baryon number) would not be probed by these measurements.

Moving beyond the scenario motivated by the CDF anomaly, we note that PV-DIS experiments possess a unique ability to probe the small parameter space for leptophobic models with axial couplings to quarks. Given the relatively large shift that may arise in this case, the observation of a significant deviation from SM expectations – coupled with the corresponding agreement of tests of the with the SM – could point strongly toward a light leptophobic scenario. Conversely, agreement with the SM would imply severe constraints on this interesting possibility.

Acknowledgements We thank J. Erler, K. Kumar, and P. Souder for helpful discussions and Y. Li and W. Marciano for sharing their input for the -dependence of the functions. This work was supported in part by DOE contract DE-FG02-08ER41531 (MJRM) and the Wisconsin Alumni Research Foundation (MJRM). MRB is supported by the US Department of Energy. Fermilab is operated by Fermi Research Alliance, LLC under Contract No. DE-AC02-07CH11359 with the US Department of Energy.

## References

• (1) P. Langacker, Rev. Mod. Phys. 81, 1199 (2009) [arXiv:0801.1345 [hep-ph]].
• (2) K. Nakamura et al. [Particle Data Group Collaboration], J. Phys. G G 37, 075021 (2010).
• (3) O. Adriani et al. [PAMELA Collaboration], Nature 458, 607 (2009) [arXiv:0810.4995 [astro-ph]].
• (4) A. A. Abdo et al. [The Fermi LAT Collaboration], Phys. Rev. Lett. 102, 181101 (2009) [arXiv:0905.0025 [astro-ph.HE]].
• (5) N. Arkani-Hamed, D. P. Finkbeiner, T. R. Slatyer and N. Weiner, Phys. Rev. D 79, 015014 (2009) [arXiv:0810.0713 [hep-ph]].
• (6) R. Essig, P. Schuster and N. Toro, Phys. Rev. D 80, 015003 (2009) [arXiv:0903.3941 [hep-ph]].
• (7) J. Erler, P. Langacker, S. Munir and E. Rojas, arXiv:1108.0685 [hep-ph].
• (8) J. Alitti et al. [UA2 Collaboration], Nucl. Phys. B400, 3-24 (1993).
• (9) M. R. Buckley, D. Hooper, J. Kopp, E. Neil, Phys. Rev. D83, 115013 (2011). [arXiv:1103.6035 [hep-ph]].
• (10) F. Yu, Phys. Rev. D83, 094028 (2011). [arXiv:1104.0243 [hep-ph]].
• (11) T. Aaltonen et al. [CDF Collaboration], Phys. Rev. Lett. 106, 171801 (2011). [arXiv:1104.0699 [hep-ex]].
• (12)
• (13) K. Cheung, J. Song, Phys. Rev. Lett. 106, 211803 (2011). [arXiv:1104.1375 [hep-ph]].
• (14) M. Buckley, P. Fileviez Perez, D. Hooper, E. Neil, Phys. Lett. B702, 256-259 (2011). [arXiv:1104.3145 [hep-ph]].
• (15) M. R. Buckley, D. Hooper, J. L. Rosner, D. Hooper, J. L. Rosner, Phys. Lett. B703, 343-347 (2011). [arXiv:1106.3583 [hep-ph]].
• (16) V. M. Abazov et al. [DØ Collaboration], Phys. Rev. Lett. 107, 011804 (2011). [arXiv:1106.1921 [hep-ex]].
• (17) E. Eichten, K. Lane, A. Martin, [arXiv:1107.4075 [hep-ph]].
• (18) M. R. Buckley, D. Hooper, J. Kopp, A. Martin, E. T. Neil, JHEP 1110, 063 (2011). [arXiv:1107.5799 [hep-ph]].
• (19) M. J. Ramsey-Musolf and S. Su, Phys. Rept. 456, 1 (2008) [hep-ph/0612057].
• (20) J. Erler and M. J. Ramsey-Musolf, Prog. Part. Nucl. Phys. 54, 351 (2005) [hep-ph/0404291].
• (21) R. W. Robinett and J. L. Rosner, Phys. Rev. D 25, 3036 (1982) [Erratum-ibid. D 27, 679 (1983)].
• (22) R. R. Subedi, X. Deng, R. Michaels, K. Pan, P. E. Reimer, D. Wang and X. Zheng, AIP Conf. Proc. 1374, 602 (2011).
• (23) Jefferson Laboratory Experiment E12-10-007, P.A. Souder (contact person), http://www.jlab.org/prog/PACpage/PAC37/ proposals/Proposals/Previously20Approved/E12-10-007.pdf
• (24) D. Boer, M. Diehl, R. Milner, R. Venugopalan, W. Vogelsang, D. Kaplan, H. Montgomery and S. Vigdor et al., arXiv:1108.1713 [nucl-th].
• (25) C. S. Wood, S. C. Bennett, D. Cho, B. P. Masterson, J. L. Roberts, C. E. Tanner and C. E. Wieman, Science 275, 1759 (1997).
• (26) S. G. Porsev, K. Beloy and A. Derevianko, Phys. Rev. Lett. 102, 181601 (2009) [arXiv:0902.0335 [hep-ph]].
• (27)
• (28) R. D. Young, R. D. Carlini, A. W. Thomas and J. Roche, Phys. Rev. Lett. 99, 122003 (2007) [arXiv:0704.2618 [hep-ph]].
• (29) K. Kumar, private communication.
• (30) S. Mantry, M. J. Ramsey-Musolf and G. F. Sacco, Phys. Rev. C 82, 065205 (2010) [arXiv:1004.3307 [hep-ph]].
• (31) T. Hobbs and W. Melnitchouk, Phys. Rev. D 77, 114023 (2008) [arXiv:0801.4791 [hep-ph]].
• (32) J. Erler, P. Langacker, S. Munir and E. Rojas, AIP Conf. Proc. 1200, 790 (2010) [arXiv:0910.0269 [hep-ph]].
• (33) J. L. Hewett, T. G. Rizzo and J. A. Robinson, Phys. Rev. D 33, 1476 (1986).
• (34) J. L. Hewett, T. G. Rizzo and J. A. Robinson, Phys. Rev. D 34, 2179 (1986).
• (35) M. Cvetic, D. A. Demir, J. R. Espinosa, L. L. Everett and P. Langacker, Phys. Rev. D 56, 2861 (1997) [Erratum-ibid. D 58, 119905 (1998)] [hep-ph/9703317].
• (36) H. Amini, New J. Phys. 5, 49 (2003) [hep-ph/0210086].
• (37) J. Erler and M. J. Ramsey-Musolf, Phys. Rev. D 72, 073003 (2005) [hep-ph/0409169].
• (38) W. J. Marciano, A. Sirlin, Phys. Rev. D29, 75 (1984).
• (39) W. J. Marciano and A. Sirlin, Phys. Rev. D 27, 552 (1983).
• (40) A. Czarnecki and W. J. Marciano, Phys. Rev. D 53, 1066 (1996) [hep-ph/9507420].
• (41) W. J. Marciano and J. L. Rosner, Phys. Rev. Lett. 65, 2963 (1990) [Erratum-ibid. 68, 898 (1992)].
• (42) S. Fanchiotti, B. A. Kniehl and A. Sirlin, Phys. Rev. D 48, 307 (1993) [hep-ph/9212285].
• (43) W. J. Maricano, ”Spin and precision electroweak physics” in the proceeding of ”XXI summer institute on particle physics: Spin Structure in High Energy Processes” (1993), SLAC-Report-444, page 35.
• (44) V. D. Barger, K. M. Cheung, P. Langacker, Phys. Lett. B381, 226-236 (1996). [hep-ph/9604298]. K. S. Babu, C. F. Kolda and J. March-Russell, Phys. Rev. D 54, 4635 (1996) [arXiv:hep-ph/9603212]. C. F. Kolda, Nucl. Phys. Proc. Suppl. 52A, 120-126 (1997). [hep-ph/9606396]; J. L. Rosner, Phys. Lett. B387, 113-117 (1996). [hep-ph/9607207]; V. D. Barger, N. G. Deshpande, K. Whisnant, Phys. Rev. Lett. 56, 30 (1986); V. D. Barger, N. G. Deshpande, J. L. Rosner, K. Whisnant, Phys. Rev. D35, 2893 (1987).
You are adding the first comment!
How to quickly get a good reply:
• Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
• Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
• Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
The feedback must be of minimum 40 characters and the title a minimum of 5 characters