Review Article  Open Access
Mathieu Buchkremer, Alexander Schmidt, "LongLived Heavy Quarks: A Review", Advances in High Energy Physics, vol. 2013, Article ID 690254, 17 pages, 2013. https://doi.org/10.1155/2013/690254
LongLived Heavy Quarks: A Review
Abstract
We review the theoretical and experimental situation for longlived heavy quarks, or bound states thereof, arising in simple extensions of the Standard Model. If these particles propagate large distances before their decay, they give rise to specific signatures requiring dedicated analysis methods. In particular, vectorlike quarks with negligible couplings to the three known families could have eluded the past experimental searches. While most analyses assume prompt decays at the production vertex, novel heavy quarks might lead to signatures involving displaced vertices, new hadronic bound states, or decays happening outside of the detector acceptance. We perform reinterpretations of existing searches for short and longlived particles, and give suggestions on how to extend their reach to longlived heavy quarks.
1. Introduction
Over the past decades, we have discovered that nature consists of a given number of elementary particles, deeply connected with the known fundamental forces driving our universe. The recent observation of a new particle resembling the longsought Higgs boson at the Large Hadron Collider (LHC) now provides us with strong evidence for the validity of the Standard Model (SM) [1, 2]. Yet, while it is generally acknowledged that the latter comprises three generations of chiral quarks and leptons, various fundamental problems do not find their answers within this framework. For instance, longstanding issues such as the origin of the fermion mass hierarchy or the nature of the CabibboKobayashiMaskawa (CKM) mixing matrix hint at the possible need for new physics. While the SM is expected to lose its predictive power as the experimental searches now reach the TeV scale, models suggesting new heavy fermions might offer solutions to these problems in the near future.
Although a fourth sequential family of quarks is now disfavoured by the recent results of the searches for the Higgs boson [3], other models predicting new heavy particles beyond the top quark are still consistent with the current experimental measurements. In particular, the possibility for vectorlike quarks, that is, quarks having their left and righthanded components transforming identically under the electroweak gauge group, is a common feature in many scenarios going beyond the SM, for example, extra dimensional models, Little Higgs models, grand unified theories, and so forth [4]. Nonchiral quarks also have the peculiarity to decouple in the heavy mass limit, leading to SMlike signals. Should the mixings of these with the light SM fermions be suppressed, the Higgs production rates would not be easily distinguishable from the SM expectations [5]. These new quarks could be sufficiently longlived to behave like effectively stable particles, evading the current searches as they propagate over sizeable distances.
From the collider searches, it is clear that if new states with masses less than a hundred GeV had existed, they would have been observed. On the other hand, the experimental reach for detecting novel heavy stable particles above the TeV scale depends on how readily identifiable such states are at the LHC. While particles with nanoseconds lifetimes could fly away from the primary interaction point before they decay to ordinary particles and lead to displaced vertices, they can also hadronise, allowing for a possibly rich spectrum of new exotic and heavy bound states. Such stable massive particles are anticipated in many new physics models, either due to the presence of a new conserved quantum number (e.g., parity in supersymmetric models) or because the decays are suppressed by kinematics or small couplings (see [6] and references therein for an exhaustive review). Although the majority of the past studies focused on stable states in supersymmetry, the possibility for new stable quarks received few attention at the LHC. While the CMS and ATLAS experiments are now setting strong limits on longlived gluino, stop and stau pair production (see, for instance, [7, 8]), scenarios involving quasistable heavy quarks have been barely investigated at the LHC.
In the following, we review the phenomenology of new, longlived heavy quarks. Assuming a general parameterisation, Section 2 first examines their production and decay modes at the LHC, considering both the chiral and vectorlike scenarios. The possible signatures for displaced vertices and stable massive hadrons are then covered within the context of negligible mixings with the SM fermions. The experimental aspects of the collider searches for new longlived quarks are presented in Section 3. We review the situation for prompt decay searches, displaced vertices, and Heavy Stable Charged Particles (hereafter, HSCPs) and highlight some of their limitations. Reinterpretations of the existing searches are then presented for short and longlived particles. Considering the possibility to improve the sensitivity of the existing analyses to longlived quarks beyond the TeV scale, some alternative search topologies are finally described. Our conclusions are given in Section 4.
2. LongLived Quarks Signatures
2.1. Production
As we review the possibility for longlived quarks in general, two different scenarios will be distinguished in this work. New chiral fermions, for which the left and righthanded chiralities have different charges under the electroweak gauge group, gain their masses from the electroweak symmetry breaking mechanism. If heavy, a sequential fourth generation quark doublet can therefore induce large corrections to loop observables. Such a scenario is now severely constrained from the electroweak precision data and the Higgs search results. Given that chiral fermions couple to the Higgs boson with a strength proportional to their Yukawa couplings, they do not decouple from its production, as the corresponding rate should increase by a factor of about 9 due to the additional fermion loops occurring in gluon fusion. The unobserved enhancement thus now strongly disfavours a fourth generation Standard Model [3].
Nonchiral quarks, on the other hand, still provide a viable extension to the SM and certainly require a dedicated discussion. Considering the introduction of new vectorlike heavy partners mixing with the SM quarks, additional parameters are allowed from invariant Yukawa interactions and Dirac mass terms in the SM Lagrangian. The light quark couplings to the Higgs and electroweak bosons are consequently modified, along with the introduction of new couplings between the heavy and the SM quarks.
Still, it is important to emphasise that such new states cannot have arbitrary quantum numbers, since they can only mix with the SM quarks through a limited number of gaugeinvariant couplings. Classifying them into multiplets, their Yukawa terms only allow for seven distinct possibilities, that is, the two singlets, the three doublets, and the two triplets displayed in Table 1.
The production of such new heavy quarks, either chiral or vectorlike, is usually assumed to proceed dominantly at the LHC through gluon fusion, . Nevertheless, depending on the model at hand, electroweak single production can also provide an alternative mechanism as it is not affected by the large phasespace suppression from which pair production suffers. In particular, new heavy quarks can be produced singly in flavourchanging processes via the electroweak interaction through , where . A comparison between the dominant production modes can be found in [10, 11] for fourth generation and in [12] for vectorlike quarks. Assuming order unity couplings, benchmark crosssections have been evaluated for various mass scenarios and reproduced in Table 2.

As described in [12], the leading contributions to vectorlike and single production arise from , , and , where denotes a valence quark parton and a generic light quark jet. Unlike QCD pair production, the above processes, however, scale with the  quark coupling squared and can be strongly suppressed if the associated mixings are negligibly small. On the other hand, Figures 2–4 in [12] indicate that falls off faster than the single production crosssections as soon as reaches the TeV scale, while the electroweak production channels displayed in Table 2 are enhanced by a factor , originating from the longitudinal polarisation of the gauge boson . Furthermore, the relative rates of the and channels strongly depend on the valence quark density in the initial state. Given the difference in the PDFs of valence and sea quarks in the initial states, new heavy quarks are produced singly at a much higher rate than antiquarks for increasing . While the quark contributes more than the quark, the neutral current contributions are weaker than the charged current ones. Finally, we underline the absence of the treelevel processes for vectorlike quarks involving exotic charges, given that they only interact with other states via treelevel charged currents [12]. Although most of the above statements are model dependent, we conclude that the large running energy of the LHC makes single electroweak production a promising discovery channel when considering new heavy quark searches with TeV/.
2.2. Decay
In the search of new fermions, the associated decay modes require careful attention. The exact partial width for a new sequential heavy quark decaying onshell to a light quark through a charged current can be written as where denotes the generic  quark coupling, equal to the CKM mixing matrix element when considering a new sequential family of quarks. Interestingly, the width (1) holds for both chiral and vectorlike singlet quarks, given that all heavytolight charged current quark decays occur to be pure  processes with identical rates [13]. If , the above partial width can be shown to reach the asymptotic form Considering a new heavy quark decaying exclusively via the above 2body decay mode, we evaluate in Table 3 the corresponding decay lengths, with GeVGeV) m and . With increasing mass, the probability for a new heavy quark to decay weakly thus becomes more and more important as its lifetime decreases. However, small couplings to the lighter SM quarks strongly affect this statement as the corresponding widths are suppressed by . As we will see in Section 2.4, this could lead to a very different phenomenology as the quarks , if very heavy, would form bound states and possibly decay hadronically.

Several conclusions can already be drawn at this stage. As far as a heavy fourth quark family is concerned, we highlight that the ratios of the charged current decay rates to the lighter families only depend on the offdiagonal mixing elements. Assuming that the extended CKM matrix is unitary, the CKM mixing elements imply nonunity branching ratios for fourth generation quarks in general.
The possibility for treelevel Flavour Changing Neutral Currents leads to similar conclusions for models involving new vectorlike quarks interacting with the SM families. Depending on their Yukawa couplings, they can undergo treelevel transitions to lighter quarks and , , and Higgs bosons. Considering vectorlike quarks with , the neutral currents and can occur with a rate of the same magnitude as given by (3), if they are allowed to mix with the light SM quarks . If no assumption is made on the hierarchy of the  coupling strengths, no exclusive decay mode to the first, second, or third family should be preferred.
For nonchiral quarks decaying to , , and , long lifetimes can be expected in the limit. Additionally, it is interesting to notice that holds in the large mass limit for most scenarios, while the chargedtoneutral current ratios approach either or depending on the vectorlike representation [14].
If more than one new heavy quark is considered, and if they are allowed to decay into each other, the partial width (3) becomes inaccurate due to the possible competition with the heavytoheavy transitions , where , depending on the model at hand. Indeed, if the decay rates of the daughter particles are significant with respect to the mass of the parent, the decay of an unstable particle is allowed through threshold effects, even if kinematically forbidden. For both chiral and vectorlike quarks, real and virtual emission near threshold proceed with the rate where [4]. While the rates essentially depend on the  quark couplings, the heavy quark mass splittings  drive the strength of the heavytoheavy transitions [11, 15]. If the quarks and belong to the same weak multiplet with a large mass splitting, the decay could be very rapid and dominate the other decay modes if there is no suppression. On the other hand, the lightest partner can only decay into an SM family quark and is thus plausibly longlived for small mixings. Should this be the case, we will see in Sections 2.4 and 2.5 that the latter could hadronize, leading to a different decay phenomenology. This occurs specifically for vectorlike singlets, which free quark decays can only proceed via nonzero mixing into the lighter generations.
As far as the doublet and triplet representations are concerned, new vectorlike partners should be very close in mass if one assumes that isospin conservation is respected. Although it may be broken by higher order corrections, such a degeneracy has been shown in [16] to require a mass difference between and MeV for nonchiral doublets, allowing for nanoseconds lifetimes. If their couplings to the lighter quarks are negligible, the partial widths for , , , and quarks are thus plausibly small.
Summarising these results, the range of the observable couplings to which longlived particle searches are sensitive at the LHC can be evaluated. From the approximation (3), the partial decay length for a vectorlike quark reads Assuming TeV/ and an experimental resolution of at least 25 m, the heavy quark decays are prompt only if their associated couplings are above the level. If , the corresponding decay lengths could be observed over a few tens of centimeters. In the limit of such small mixings with the SM fermions, it is thus natural to motivate searches for displaced vertices.
2.3. Classification of Signatures
We now detail the possible situations giving rise to the observable signatures of longlived quarks at the LHC.
The classification given in Table 4 summarises the longlived quark scenarios corresponding to the small mixing scenarios treated in this work. We emphasise that if mixing with all SM quark families is permitted, direct searches should aim at being sensitive to all light quarks in the observed final states. Given that their interactions are allowed through arbitrary Yukawa couplings, the searches for longlived vectorlike quarks should be as inclusive as possible in order to cover the full spectrum of possibilities at the LHC. Such a program is important to set new constraints on the decay modes, independently of any assumptions on the  mixing sector. The relative importance of the channels is most relevant compared to the charged currents, as no exclusive decay mode should be preferred for .

As illustrated in Figure 1, three cases for new longlived quarks can be distinguished depending on their mixing parameters with the SM fermions. (i)Firstly, if all couplings with the known SM fermions are larger than the level, all heavytolight decays are prompt, over distances smaller than 25 m. This defines the shortlived scenario (i), with no experimental difference compared to the direct searches.(ii)The second scenario (ii) arises for intermediate decay lengths ranging between a few microns and centimetric distances. If there is at least one light quark such that , displaced events could be observed, yet with a partial width suppressed by . Consequently, if all the couplings but one are below the level, a single exclusive channel would lead to a prompt decay signature corresponding to a shortlived heavy quark. A possible exception, though, is the case for new heavy multiplets with sizeable mass splittings, as allowed in extra generation models and possible extensions [11, 17–19]. If , the heaviest quark can be shortlived and decay semiweakly to , while the lightest partner is likely stable if all its decay modes suffer severe suppression. If , on the other hand, all heavytoheavy transitions are suppressed and both quarks could be longlived on detector scales. (iii)For particles with decay lengths larger than the detector dimensions lies the longlived region (iii), the details of which will be discussed in Section 2.4. If all heavy quark couplings with the SM fermions are below the level, the stable case becomes a relevant scenario, possibly in conjunction with displaced events.
We emphasise that the scenarios for which prompt decays and displaced vertices could be observed only call for one of the allowed decay modes to fulfill the associated conditions. The stable scenario, however, requires all decay lengths and partial widths to lie in the ranges given in Table 4. As we will see in Section 2.4, if all  quark couplings to the SM families are smaller than , such new heavy fermions could hadronise. As a result, the annihilation decays and hadronic transitions between the formed bound states would dominate, while the single quark decay events might be suppressed.
2.4. Signatures for Heavy Stable Particles: Heavy Quarkonia
Previously, we have discussed how displaced events could occur in the single quark decay transitions in the case of small  couplings. In this section, we describe the possibility for new heavy quarks to bind into hadrons if their lifetime is large enough, providing us with an interesting alternative for new signal searches at the LHC.
While new coloured particles with masses heavier than the top quark are usually assumed to decay as free particles, their possible formation into baryons and mesons is an important issue to consider in the case of small couplings with the SM fermions.
Should the partial widths be suppressed, the quark might be stable and hadronise. Assuming that the binding force in a fourth generation bound state is of Coulombic nature, the seminal condition was derived in [20] for () formation. According to (6), new heavy quarks form hadronic states if their mixing with known quarks is sufficiently small. Mixings roughly smaller than 0.2 are typically required for GeV/ new quarks to form bound states, which remains perfectly consistent with the current bounds from the electroweak precision observables. As shown on Figure 2 for a new uplike fourth generation quark , the electroweak precision fits typically restrict the mixing matrix element to be smaller than for GeV/. If lighter, the total width can be smaller than MeV [11], thus allowing new chiral quarks to form bound states with nanosecond lifetimes.
As far as nonchiral fermions are concerned, the electroweak precision constraints provide upper bounds on the mixing parameters, but are not as restrictive given that their effects decouple in the limit of large masses [21]. Although vectorlike quarks are usually considered to couple dominantly to the heaviest third quark family (see [12, 22] for some exceptions), they are allowed, in principle, to mix with all up (down) type quarks [14].
In any case, is used as a rule of thumb in most of the allowed vectorlike representations [14]. Furthermore, corrections to the CKM matrix elements are required to be small for singlets [23], doublets, and triplets [24]. In this framework, the hadronic production of new bound states involving sequential or nonchiral quarks is a conceivable possibility at the LHC. Assuming that (6) is satisfied due to small  couplings, their lifetime can be longer than the orbital period of the corresponding () bound state, allowing to build up new quarkonium resonances, openflavour mesons, and baryons [20].
If their formation is governed by the same strong interactions that are responsible for the existence of the ordinary hadronic spectroscopy, the associated mass spectrum can be determined from the known properties of lowenergy hadron physics [25]. Considering a simplified model of QCDlike hadrons, new heavy quarks would form bound states (hereafter defined as ) from induced, strongly attractive potentials. Conjointly, quarkonium formation can arise from Higgs boson exchange, as the corrections from Yukawatype forces cannot be neglected for large quark masses [26, 27]. In [28], Hung detailed the numerical resolution of a general nonrelativistic Higgs exchange potential, with interesting consequences on the associated scalar spectrum. More recently, Enkhbat et al. gave a preliminary discussion of the fourth generation Yukawa bound states phenomenology at the LHC, considering an ultraheavy degenerate new quark family [29]. Although binding energies of Yukawa origin certainly provide a more consistent framework for a dedicated analysis, we restrict the present discussion to the context of Coulomblike potential models and assume that the shortdistance behaviour of the quarkantiquark potential dominates (we refer the reader to [30, 31] for previous and more exhaustive phenomenological reviews). In this context, the effects of the quarkonium wave function must be taken into account as we consider the corresponding production and decay modes. In perturbative QCD, the dominant contribution to production crosssection in collisions reads [30] where , and denotes the gluon luminosity with . The full NLO partonic crosssections for the , , and initiated reactions are provided in [32] and have been updated in [33]. Interestingly, they are all proportional to the square of the radial wave function at the origin, which might drive the heavy quarkonium production crosssection to be substantially smaller than . Indeed, the quarkonium production rate typically amounts to a few percent of the pair production crosssection [32–34].
Depending on whether the decay rate of the constituent particles, , is larger or smaller than the bound state annihilation rate, two different cases that can be considered as the bound states can either undergo single quark decays or annihilate hadronically. As detailed in [35], the strength of the annihilation decay signal is enhanced when the intrinsic width of the heavy quark is decreased. Should its rate be of the same order of magnitude as the binding energy of the state, the quarkonium can be broad and display little evidence of any resonance behaviour over the continuum. On the other hand, if its 2body decays are suppressed due to kinematical suppression or small couplings as discussed in Section 2.2, can only decay through offshell intermediate states. In such a case, the signature would correspond to an annihilation signal, namely, a hadronic final state markedly distinguishable from pair production and decay.
We now give a brief and qualitative description of some of the expected hadronic signatures at the LHC, considering either a chiral or vectorlike heavy quark . While similar results hold for all  and wave quarkonium states, we limit our analysis to the case of a stable, neutral pseudoscalar state . In particular, an quarkonium state formed from downtype fourth generation quarks is known to provide a possible candidate if the condition (6) is satisfied [33]. The latter is mainly produced through the gluon fusion process (8) with a production crosssection two orders of magnitude larger than the vector state [33]. If is the lightest fourth generation quark, a bound state can decay either through  family mixing with , or to boson pairs. Whether the single quark decays would compete with the hadronic modes depends on the heavy quark masses and mixings. If TeV/, a fourthgeneration downtype quark dominantly decays into fermionantifermion pairs if . For TeV/, the total width lies below GeV/, and the quarkonium state decays proceed dominantly via the annihilation diagrams depicted in Figure 3 [33]. Decays to gauge boson pairs, fermionantifermion pairs, gaugeHiggs, and Higgs boson pairs can occur through , and exchange in the channel or proceed via quark mixing in the  and channels, if allowed. Decays to Higgs boson pairs () are forbidden by CP conservation in the case of pseudoscalars. While the processes involving charged currents are suppressed in the case of small quark couplings, the mode is allowed at looplevel via the exchange of the partner , even if . Decays to pairs are not allowed for bound states involving singlet vectorlike quarks.
(a)
(b)
(c)
(d)
(e)
An exhaustive study of the production and subsequent decays of the  and wave quarkonium states of a heavy chiral quark is available in [30, 36], where all the allowed production mechanisms and decay patterns have been thoroughly investigated. As an illustration, we compare in Figure 4 the branching ratios of the allowed decay modes for quarkonium states formed by a chiral fourth generation quark and a vectorlike isosinglet quark [36]. The quarkonium annihilation decay rates depend markedly on the mass scale.
(a)
(b)
In the chiral case, the main decay modes are , , , , , and , respectively. The fermionic decays are also allowed if . Substantial decay rates to fermion pairs are allowed in case of large  couplings. For pseudoscalar masses lighter than GeV/, the dominant annihilation mode proceeds via the strong interaction, that is, . For larger masses, the width into two gluons is decreasing, whereas the annihilation mode into pairs takes over. This follows from the fact that the decay rates into Higgs and longitudinal gauge bosons are enhanced by the large Yukawa coupling of the heavy quark, so that the branching ratio becomes sizeable for increasing masses. The latter channel then leads to a salient signature for heavy fourth generation bound states.
While fourth generation pseudoscalar quarkonia decays allow for striking signals, and bound states of vectorlike quark singlets can only decay to , , , and pairs, as the mode is absent [36]. This follows from the fact that the mode proceeds through the axial part of the neutral current coupling, which in turn is proportional to the third component of the weak isospin. Only , , and would then signal the visible hadronic modes with branching ratios of about . and bound states of vectorlike singlet quarks are thus hardly observable at the LHC as the gluon mode dominates. On the other hand, and vectorlike doublet (triplet) partners with nonvanishing weak isospin can have large branching ratios to via , , or exchange in the channel. The and quarkonia provide a noticeable exception, given that the exotic quarks and do not couple to neutral currents at tree level. Since they only mix with the other states via charged currents, the annihilation modes including , , and exchange are thus forbidden for and , which then mainly decay to and bosons. Although it is suppressed below the percent level, the distinctive diphoton decay mode also provides a possible golden channel for discovery. If new stable, coloured particles are produced at the LHC, the resulting final states could indeed allow for resonant signatures including photons and leptons, from which their quantum numbers and masses can be identified independently of their decay modes. As the decay rate for such bound states might be small, modelindependent searches for new resonances could be competitive with the direct searches [35].
2.5. Signatures for Heavy Stable Particles: OpenFlavour Mesons
While quarkonium resonances might be challenging to observe, the possibility for “openflavour” hadrons () and (), with being a light SM quark, also covers a broad spectrum of new heavy mesons and baryons to search for. Should they be produced at the LHC, such states can form by capturing a light quark partner from the vacuum. As they pass through the detector, they can transform into various slowly moving heavy states. Assuming that they hadronise with , , and quarks after being produced, Table 5 lists the corresponding allowed stable mesons and baryons.

The properties of new hypothetical fourth generation quarkonium and openflavour mesons have been examined previously in [37] considering large expansion techniques. In [38], their masses and decay constants have been estimated from the experimental measurements of the ordinary () hadron masses, using the QCD sum rules. Interestingly, both approaches indicate that the corresponding spectra share numerous features with most of the scenarios predicting stable bound states of heavy quarks beyond the Standard Model, depending on their masses, charges, and angular momenta.
Interestingly, the interactions of such openflavour mesons with the material occur to be similar to those of hadrons, that is, stable hadrons composed of a supersymmetric particle and at least one SM quark (see [39, 40] and references therein for related works). The 1/2 difference in spin with respect to stop hadrons has little impact on the search strategies, which depend mostly on the interactions between the lighter quarks and the matter of the detector. This is in substance the description given by the spectator model [41, 42], for which the allowed transitions of heavy and light quarks within a given bound state are known to be flavour and spin independent [43, 44]. In this context, the heavy quark can be considered as a source of kinetic energy of which sole function is to give mass and momentum to the underlying hadron. Such new heavy bound states then behave as rather passive objects, consisting of a noninteracting heavy component, accompanied by lighter constituents ( and quarks, mostly). While the partons are being scattered within the detector, their crosssections vary with their inverse mass in perturbative QCD [6, 25]. A heavy () bound state is then expected to suffer small energy losses when interacting with the material, given that only its light quark half is responsible for the hadronic interactions with the detector.
We list in Table 6 the various allowed and transitions involving mesontomeson and mesontobaryon conversions. In general, these interactions lead to simultaneous pion emission as the initial mesons convert into slowly moving baryons.
(a)  
 
(b)  
 
(c)  
 
(d)  

While they interact with the nuclear matter, most of the new states suffer multiple scattering and convert into baryons, allowing for , , and states, as new heavy mesons are kinematically favoured to increase their baryon number by emitting one or more pions [25]. Due to the lack of these in the material, the reverse reaction is known to be less favoured.
Interestingly, new mesons which convert at the beginning of the scattering chain could generate tracks with “dashedlines,” signalling possible baryonic or electric charge exchange. Indeed, and bound states traversing a medium composed of light quarks likely flip their electric charge, frequently interchanging their parton constituents with those of the material nuclei. Eventually, they could leave the detector as heavy stable neutral particles and hence not be observable in muon detectors. The modeling of the nuclear interactions of new heavy hadrons traveling through matter, a survey of which is given in [25, 45], actually favours scenarios with significant charge suppression if heavy openflavour mesons have a sizeable probability to transform into neutral particles while traversing the detector. This poses a serious challenge for the experimental searches, since the most conservative scenarios assume a complete charge suppression where 100% of the produced hadrons become neutral before reaching the muon detectors. Taking a specific example, we consider pairproduced quarks hadronising into the heavy states and immediately after production. For convenience, we assume that a majority (≳90%) of the new heavy quarks initially hadronise into mesons, while a smaller amount (≲10%) form baryons [6]. As they interact farther in the detector, most of the mesons eventually exit the detector as and mesonic states, or as baryons. Baryontomeson conversions are allowed as well, as these states can also annihilate back into and mesons, yet with a smaller rate. mesons of vectorlike antiquarks, on the other hand, unlikely give rise to antibaryons, but can still flip their charge through the exchange of and quarks with the material. Possibly large flavour fractions for and can thus be expected in the detector, with a negligible amount of states. If such antibaryons were to form, they would quickly annihilate by baryontomeson interactions, producing pions [46].
After travelling through the detectors a few nuclear lengths away from the production vertex, the novel hadrons transform in roughly 100% to the positively charged baryon , whereas one half of the states thus transform into mesons, and the other half in . The corresponding hadronic flavour decompositions, evaluated as a function of the penetration depth in the detector, can be read from Figure 5 of [25] for hadrons involving stable scalar top and antitop quarks. We notice that similar results are obtained when replacing stop squarks by stable quarks of equal mass. The , (), and (), states are then expected to retain the largest flavour composition fractions when considering penetration depths larger than meters and are thus the most likely observable states, which we emphasised in bold font in Table 5.
Except for and , it is interesting to notice that none of the states listed in Table 5 is neutral if involving vectorlike quarks with exotic charges. The corresponding bound states might give rise to possibly large fractions of slowly moving charged particles and with and , respectively, accompanied by a small amount of , , , and mesons (and charge conjugates). These particles are all electrically charged as they go across the detector, emitting charged and neutral pions in the process together with losing small amounts of energy. Given the small expected interaction crosssection from the MesontoBaryon transitions, the processes shown in Table 6 leave small energy deposits in the calorimeters, of the order of GeV [6]. On the other hand, such stable hadrons would lead to observable tracks due to the ionisation energy losses, allowing for signatures similar to slowmoving muons with high transverse momentum. Searches for stable charged particles, if adapted to such a case, thus provide a promising strategy to rule out the possibility for novel exotic quarks with large lifetimes. Given these very specific signals, the aforementioned signatures can certainly be discriminated at the LHC.
3. Experimental Aspects
In this section, we review the past and current experimental searches for new longlived quarks. Limitations of these searches are then discussed along with possible extensions to enhance sensitivity to heavy quarks. Reinterpretations of direct searches for heavy quarks as well as general searches for longlived particles are given in the context of longlived heavy quarks.
3.1. Previous Searches at Tevatron
The searches undertaken at the Tevatron resulted in already stringent mass bounds on longlived heavy quarks, yet not without assumptions. Looking for longlived parents of the boson in displaced vertices from collisions at TeV, CDF set limits on the crosssection of a fourth generation charge quark as a function of its lifetime with an integrated luminosity of [47]. Isolated electronpositron pairs originating from decays were searched for in the exclusive channel with . Finding no evidence for new longlived particles, CDF excluded GeV/ for 1 cm at 95% CL. This limit drops to GeV/ if 22 cm or 0.009 cm. Previously, the D0 collaboration already ruled out the range from searches in [48] for all proper lifetimes, while a quark with a mass lower than was previously dismissed by the LEP direct searches [49]. Within a 90 data sample of collisions recorded during 19941995, CDF performed a search for low velocity massive charged stable particles leaving large amounts of energy in the calorimeters [50].
Assuming a muonlike penetration and searching for an anomalously high ionisation energy loss signature, the data was found to agree with background expectations, and upper limits of the order of 1 pb were derived on the production crosssection. Sensitive to longlived fourth generation quarks scenarios, the lower bounds GeV/ and GeV/ have been obtained for and stable quarks, respectively, with no observed excess over background. More recently, D0 studied a 1.1 data sample and looked for decays assumed to follow from a longlived quark parent with BR( [51]. Assuming that the electromagnetic showers were originating from the same vertex, the analysis found no hint away from the interaction point. D0 excluded GeV/ at the 95% confidence level for decay lengths between 3.2 mm and 7 m. With the same integrated luminosity, CDF excluded GeV/ at 95% CL, considering a longlived quark decaying exclusively into a boson and a jet [52]. However, it has been emphasised in [53] that the assumption BR( is inaccurate for GeV/, given that the decay mode should take over if . Furthermore, the processes were hinted to proceed with nonnegligible rates, leading to an even lower branching ratio. Indeed, even if the decay dominates, the aforementioned mass limits depend sensitively on the CKM mixing elements between the fourth and the first three generations. If nonunity couplings between the fourth and the lighter quarks are allowed, the CDF lower bound on can be significantly affected.
Additionally, it is known that the above CDF limits do not apply for longlived heavy quarks decaying between roughly 1 cm and 3 m within the detector [53]. Should their couplings to SM quarks lie in the corresponding range –7, there exist no bounds on the and masses in this uncovered region. For decay lengths larger than the detector dimensions, the lower bounds drop to GeV/ and GeV/, as obtained from the stable quark searches [50, 51].
3.2. LHC
3.2.1. Limitations of Direct Searches
While dedicated results for longlived bound states of vectorlike heavy quarks are still missing at the LHC, various searches for heavy quarks of zero lifetime have already been performed by the ATLAS and CMS experiments. In this section, we discuss how the results of searches for prompt production could be reinterpreted for lifetimes larger than s.
The main aspects of reinterpreting these results are the branching ratios to the investigated final states, which may be different in alternative models, and of course the lifetime of the heavy particle.
Considering here a specific example, the current best limit on production, published by the CMS collaboration, excludes production crosssections of pb at 95% CL with an integrated luminosity of 4.9 at TeV [54], assuming a branching ratio . As we have seen in Section 2.2, the assumption of exclusive branching ratios is not generally valid for new heavy quarks. Nevertheless, the fraction to which a hypothetical signature occurs can be used to recalculate the crosssection limit in the most naïve approximation where is the excluded crosssection under the assumption of BR_{assumed} and BR_{true} is the branching ratio in the given model.
While this statement is a trivial estimation, the reinterpretation for longer lifetimes requires more thought. In particular, the implicit assumption of heavy quarks decaying promptly at the production vertex is valid only for very short lifetimes. If these particles form bound states and propagate certain distances before their decay, they can potentially escape the direct searches. In such a scenario, the published limits could be considerably weaker, depending on the particle’s lifetimes, simply because they would fly too far to be detected at the primary vertex.
For intermediate lifetimes with displaced decay vertices within the detector volume (cf. the region (ii) discussed in Section 2.3), a recalculation of the published limits can be attempted. Assuming an exponential decay function, a fraction of the decays will always happen in the vicinity of the beam line, so that the prompt searches will pick them up. Based on this fraction, one can recalculate the limits as a function of the heavy quark lifetime. However, in order to do this correctly, one requires the exact selection efficiency as a function of the displacement from the beam line. Unfortunately, such information has not been made available by the experiments. Still, it can be estimated from an educated guess under specific assumptions. For instance, the analysis in [54] applies jet tagging, which requires highquality tracks to originate within the inner detector volume. The CMS innermost part, the pixel detector consists of three barrel layers with the innermost layer at a distance of cm from the beam line. This represents the technical limitation to this analysis, so that we can assume that the selection efficiency vanishes at a transverse displacement of around cm.
Even in analyses without application of jet tagging, stringent quality cuts are usually required to select reconstructed detector objects originating from the primary vertex. One of the motivations for these requirements is the rejection of pileup. Jets from displaced decays which do not point to the production vertex are mostly removed by the pileup cleaning procedures. We therefore make the assumption that events are kept in the direct searches if the decay happens at less than cm from the primary interaction vertex, and lost otherwise. The fraction of the lost events can be determined from the distance that these particles travel before their decay. This distance depends on the mass, the momentum, and the proper lifetime . It is defined in the laboratory frame as . The fraction is obtained by convoluting with an exponential decay function and the momentum spectrum which determines and .
We take the momentum spectrum of pairproduced heavy quarks as predicted by the MadGraph [55] Monte Carlo generator. The assumed center of mass energy is TeV. The momentum is needed for a precise calculation of the decay distance on an event by event basis because the velocity may be significantly smaller than . The distribution for various quark masses is shown in Figure 5. The distribution of the velocity in units of is shown in Figure 6.
Our simulation assumes that the production mechanism and kinematics are independent of the lifetime of the particle. Possible limitations of that assumption are discussed in Section 3.2.4. Calculating the distribution of decay vertices in the detector frame, we obtain the fraction of decays outside of the geometrical acceptance of cm as a function of the proper lifetime . Table 7 summarises our results for four benchmark points in the parameter space. The results are displayed as a function of the proper lifetime in Figure 7.

We conclude that direct searches are only valid for lifetimes which are considerably shorter than about s; otherwise the particles would propagate too far and be rejected by the selection criteria. We also stress that this result is relatively independent of the particle masses within our approximations.
The published limits on the heavy quark production crosssections can be simply reinterpreted in the region s s by where is the fraction of lost events given in Table 7 and Figure 7. The recalculation of the mass limits can then be done by comparing the recalculated crosssections with predicted crosssections as a function of the mass.
3.2.2. Displaced Vertices
The immediate question that arises from the previous results is whether lifetimes larger than s are covered by dedicated searches for longlived particles, either through displaced vertices or signatures of stable particles propagating through the full detector.
Displaced topologies have been searched for at LHC and published, for instance, in [56, 57]. These searches are indirectly applicable to heavy quarks and will be discussed in this section.
The CMS analysis [56] is looking for massive longlived spinless neutral bosons, produced in decays of Higgs bosons (). The bosons are decaying to dileptons . This analysis is feasible thanks to the CMS track reconstruction algorithm which is able to identify very displaced tracks not originating from the primary interaction vertex. By fitting tracks of two oppositely charged leptons to a common vertex, transverse displacements up to cm from the beam line can be reconstructed. This analysis is very sensitive, and it is able to put limits on production crosssections of the order of pb at 95% CL, depending on the assumed masses of the bosons and their mother particles. The decays of heavy quarks such as , for instance, can lead to displaced dilepton vertices as well, because both bosons can decay leptonically.
In this analysis, the momentum of the vertex is required to be parallel to the vector pointing from the primary vertex to the boson decay vertex in the transverse plane. This “collinearity” cut is 0.2 (0.8) radians for muon (electron) final states. A direct interpretation of the published limits in context of longlived heavy quarks is therefore not straightforward. Due to the presence of the neutrinos and of the quark jet in decays, the momentum of the dilepton vertex will not be parallel to the vector pointing from the primary to the secondary vertex. However, we can attempt to estimate the efficiency of this collinearity cut based on simulated events. We use again our MadGraph simulation from Section 3.2.1 and calculate the angle between the momentum of a heavy quark and the dimuon momentum in leptonic decays. It is found that the distribution of this collinearity angle is fairly independent of the mass of the heavy quark. The collinearity cut has an efficiency of 68% for electrons and 25% for muons in leptonic decays which represents a moderate decrease. A reinterpretation of the published results, taking these efficiencies into account, will be considered in the following.
A central component that would be necessary to derive trustworthy limits on heavy quark production from displaced vertex searches is the Monte Carlo simulation of the signal process. The interactions of these heavy particles with the detector material and the efficiency of their reconstruction and selection need to be estimated in order to facilitate the calculation of limits. Difficulties may arise from missing implementations of certain exotic models in the simulation software. Existing simulations of heavy stable particles such as those of hadrons may provide good approximations though [25].
We see in [56] that different assumptions for the masses and lead to different exclusion limits due to the kinematical properties of the final state. A direct matching of the mass of a heavy quark to and is not straightforward. The assumption that the results from [56] are applicable for heavy quarks can therefore only be understood as an approximation. In the following we assume that the limits for higher and values are more applicable to heavy quarks, so we only consider those mass points with GeV/ and GeV/. Fortunately, the resulting exclusion limits vary only in a small window between pb and pb in the dimuon channel for cm cm when scanning the various mass points for and . Following the strategy of a worst case scenario we use the worst limit of pb which weakens to pb taking the effect of the collinearity cut into account. Now the final state has only a 1% branching ratio into dimuons which results in an excluded crosssection of pb for cm cm. In the context of QCD pair production of heavy quarks, the value of 0.8 pb corresponds to a mass of GeV/ at TeV [58]. This can therefore be assumed to be the exclusion limit under the assumption of a branching fraction . Comparing this to the searches at CDF and D0 quoted in Section 3.1, we see a clear improvement of the limits, at least in the range cm cm. While the reinterpretation is difficult due to the discussed reasons, much stronger bounds would certainly be possible by including the heavy quark signatures into the displaced vertex analysis.
A displaced vertex analysis has also been performed by the ATLAS collaboration [59], following a slightly different strategy. Displaced vertices are reconstructed in an inclusive way, using all displaced tracks in the event as potential seeds. In contrast to CMS, where only oppositesign dimuon vertices have been used, the ATLAS approach requires at least five tracks at the vertex and an invariant mass of the vertex of at least 10 GeV/. To ensure a good fit quality, only vertices within the fiducial barrel pixel detector volume are considered, which means that transverse displacements up to cm are considered. In addition, one muon with GeV/ is required to be associated with the signal vertex. This analysis has been carried out in the context of an parity violating supersymmetric scenario, deriving limits on , where is the square of the branching ratio for produced squark pairs to decay via longlived neutralinos to muons and quarks. The requirement that the triggering muon candidate is associated with the displaced vertex ensures that the selection efficiency for each neutralino is independent of the rest of the event. This facilitates a reinterpretation for scenarios with different numbers of longlived neutralinos in the event.
Also in this analysis the limits depend on masses and kinematics of the hypothetical longlived particles and their mother particles. In the most pessimistic scenario the excluded crosssections are approximately pb for lifetimes of 3 mm mm using an integrated luminosity of 4.4 at TeV. For even larger lifetimes of mm mm the limits are better than pb.
The interpretation of these results for decays such as the or even is possible because these signatures would certainly give rise to decay vertices with very high invariant mass and high track multiplicity. The final states have at least one muon in 19% of the cases which means that the excluded values are pb for 3 mm mm. This is about an order of magnitude better than our reinterpretation of the CMS result. The value of 0.05 pb corresponds to GeV/ [60].
3.2.3. Heavy Stable Charged Particles
For very longlived scenarios (cf. the region (iii) discussed in Section 2.3), the new heavy states do not decay, but they travel through the full detector. In the following we review recent results by CMS [61] along with an assessment of their relevance for HSCPs.
The main identification criteria for HSCPs are high momentum, high ionization, and long time of flight (TOF). The energy loss along the track is calculated from the charge deposits in the silicon tracker, while the TOF is obtained from the arrival time in the muon system. These quantities are uncorrelated for SM particles. This noncorrelation is used to estimate the background yields in signaldepleted regions.
Models of charge suppression due to interaction of HSCPs with the detector material are considered as well. If charged particles become neutral while propagating through the detector they do not reach the muon chambers. The TOF criterion cannot be used in this case. Therefore, the results have also been estimated without the TOF requirement at the cost of weaker exclusion limits.
The obtained limits for a given mass can be very different depending on the assumed particle type. This is due to the predicted kinematics of the particle and its expected detector signal. For instance, the limit on pair production of a scalar top quark with a mass between and GeV/ is 3 fb for an integrated luminosity of at TeV.
Limits for longlived heavy quarks have not been considered explicitly, unfortunately. However, as an approximation, we make the assumption that a longlived bound state of a stop would behave similar or equal to a bound state of a heavy uptype quark [25]. This concerns both the interaction with the detector material and the production mechanism which is assumed to proceed via the strong interaction. It is then possible to use the stop exclusion limits directly for stable heavy quarks. Limitations in that assumption are discussed in Section 3.2.4.
The predicted production crosssections of heavy quarks are quite large for low masses (Section 2.1). Even with a large systematic safety margin, these crosssections can be considered to be excluded by the HSCP searches. The heavy quark pair production crosssection for GeV/ (the highest mass value considered in [61]), computed at NLO, is fb at TeV [58], which can therefore be assumed to be excluded for sufficiently long lifetimes. Heavy quark masses of the order of TeV/ are not yet excluded though, neither in direct searches for prompt decays nor in longlived searches.
To make a quantitative statement about the excluded lifetimes by the HSCP searches, we repeat our simulation from Section 3.2.1. To be detected by these analyses, the particles have to be produced at the primary vertex and they have to traverse the full tracking devices, and the muon chambers for the combined trackeOF analysis (or the tracker for the trackeronly analysis). The CMS tracker has a length of about m and a diameter of m [62]. We can calculate the fraction of decays inside the tracker volume and assume that these decays will not be reconstructed in the HSCP analyses because of missing hits in the outermost tracker layers.
Table 8 and Figure