An SLC-type $e^{+}e^{-}/\gamma\gamma$ facility at a Future Circular Collider

It is proposed to place the arcs of an SLC-type facility inside the tunnel of a Future Circular Collider (FCC). Accelerated by a linear accelerator (linac), electron and positron beams would traverse the bending arcs in opposite directions and collide at centre-of-mass energies considerably exceeding those attainable at circular $e^{+}e^{-}$ colliders. The proposed SLC-type facility would have the same luminosity as a conventional two-linac $e^{+}e^{-}$ collider. Using an optical free-electron laser, the facility could be converted into a $\gamma\gamma$ collider. A superconducting L-band linac at the proposed facility may form a part of the injector chain for a 100-TeV proton collider in the FCC tunnel. The whole accelerator complex would serve as a source of $e^{+}e^{-}$, $\gamma\gamma$, $pp$ and $ep$ interactions. The L-band linac could also be used to produce high-intensity neutrino, kaon and muon beams for fixed-target experiments, as well as X-ray free-electron laser (XFEL) photons for applications in material science and medicine.


Introduction
The Standard Model (SM) of particle physics gives a coherent quantum-mechanical description of electromagnetic, weak and strong interactions based on fundamental constituents -quarks and leptons -interacting via force carriers -photons, W and Z bosons, and gluons. The SM is supported by two theoretical 'pillars': the gauge principle and the Higgs mechanism for particle mass generation. In the SM, where electroweak symmetry is broken by the Higgs mechanism, the mass of a particle depends on its interaction with the Higgs field, a medium that permeates the universe. The photon and the gluon do not have such couplings, and so they remain massless. The SM predicts the existence of a neutral spin-0 particle associated with the Higgs field, but it does not predict its mass.
Whereas the gauge principle has been firmly established through precision electroweak measurements, the Higgs mechanism is yet to be fully tested. A state decaying to several distinct final states was observed in 2012 at the CERN Large Hadron Collider (LHC) with a statistical significance of five standard deviations [1,2]. The observed state has a mass m H ≈ 125 GeV. Its production rate is consistent with the predicted rate for the SM Higgs boson. Furthermore, event yields in different production topologies and different decay modes are self-consistent [3].
All of the couplings of the Higgs particle to gauge bosons and fermions are completely determined in the SM in terms of electroweak coupling constants and fermion masses. In the SM, Higgs production and decay processes can be computed unambiguously in terms of the Higgs mass. Since the coupling of the Higgs boson to fermions and gauge bosons is proportional to the particle masses, the Higgs boson is produced in association with heavy particles and decays into the heaviest particles that are kinematically accessible.
The Higgs-boson mass affects the values of electroweak observables through radiative corrections. Many of the electroweak measurements obtained over the past three decades may be combined to provide a global test of consistency with the SM. The best constraint on m H is obtained by making a global fit to the electroweak data. Such a fit strongly suggests that the most likely mass for the SM Higgs boson is just above the limit of 114.4 GeV set by direct searches at the LEP e + e − collider [4]. This is consistent with the value of the Higgs mass measured at LHC.
High-precision electroweak measurements, therefore, provide a natural complement to direct studies of the Higgs sector. All the measurements made at LEP and SLC could be repeated at the proposed facility using 90% polarized electron beams and at much higher luminosities [5].
The rich set of final states in e + e − and γγ collisions at the proposed SLC-type facility would play an essential role in measuring the mass, spin, parity, two-photon width and trilinear selfcoupling of the SM Higgs boson, as well as its couplings to fermions and gauge bosons. Such measurements require centre-of-mass (c.m.) energies √ s ee < ∼ 600 GeV, considerably exceeding those attainable at circular e + e − colliders.

2
Single SM Higgs production in e + e − annihilations A particularly noteworthy feature of an e + e − collider is that the Higgs boson can be detected in the Higgs-strahlung process (see Fig. 1) even if it decays into invisible particles (e.g., the lightest neutralino of a supersymmetric model).
In this case the signal manifests itself as a peak in the invariant mass distribution of the system which recoils against the lepton pair stemming from Z-boson decay. In Eq. (1), λ HZZ is the Higgs coupling to the Z boson and s ee is the square of the c.m. energy. By exploiting the HZ → Xℓ + ℓ − channel, the Higgs-strahlung cross-sections can be measured with a statistical error of about 2 percent for a Higgs-boson mass m H ≃ 125 GeV (see [6] and references therein). From the fits to the reconstructed mass spectra in the channels HZ → qqℓ + ℓ − , bbqq, WWℓ + ℓ − and WWqq, the Higgs-boson mass can be determined with an uncertainty of about 40 MeV for m H ≃ 125 GeV [6].
To determine the spin and parity of the SM Higgs boson in the Higgs-strahlung process, one can use the information on (1) the energy dependence of the Higgs-boson production cross-section just above the kinematic threshold, and (2) the angular distribution of the Z/H bosons. The best way to study the CP properties of the Higgs boson is by analyzing the spin correlation effects in the decay channel H → τ + τ − [6].
The Higgs-strahlung cross-section, which dominates at low c.m. energies, decreases with energy in proportion to 1/s. In contrast, the cross-section for the W-fusion process (see Figs 1 and 2) e + e − → Hνν, σ(e + e − → Hνν) ∝ λ 2 HWW log(s ee /m 2 H ) (2) increases with energy in proportion to log(s ee /m 2 H ), and hence becomes more important at energies √ s ee > ∼ 500 GeV for m H ≃ 125 GeV. In Eq. (2), λ HWW is the Higgs coupling to the W boson.
The Higgs-fermion couplings can be extracted by measuring the branching fractions of the Higgs boson. There are two methods to determine the Higgs branching fractions: (1) Measure the event rate in the Higgs-strahlung process for a given final-state configuration and then divide by the total cross-section; (2) Select a sample of unbiased events in the Higgs-strahlung recoil-mass peak and determine the fraction of events that correspond to a particular decay channel. See [6] and references therein for an estimate of the accuracy that can be achieved in such measurements.
For m H < 2m W , the total decay width of the Higgs boson, Γ H , can be determined indirectly by employing the relation between the total and partial decay widths for a given final state: For instance, consider the decay H → WW * . One can directly measure the branching fraction BR(H → WW * ), determine the coupling HZZ in the process e + e − → HZ, relate the HZZ and HWW couplings (λ HZZ /λ HWW = m 2 Z /2m 2 W ), and then use the fact that Γ(H → WW) ∝ λ 2 HWW to obtain the partial width Γ(H → WW * ) from the information on the HWW coupling. The accuracy with which the determination of Γ H can be achieved for m H ≃ 125 GeV is estimated in [6].   Single SM and MSSM Higgs production in γγ collisions Since photons couple directly to all fundamental fields carrying the electromagnetic current (leptons, quarks, W bosons, supersymmetric particles), γγ collisions provide a comprehensive means of exploring virtually every aspect of the SM and its extensions (see [9,10] and references therein). The cross-sections for production of charged-particle pairs in γγ interactions are approximately an order of magnitude larger than in e + e − annihilations. For some processes within and beyond the SM, the required c.m. energy is considerably lower in γγ collisions than in e + e − or proton-proton interactions.
In γγ collisions, the Higgs boson is produced as a single resonance in a state of definite CP, which is perhaps the most important advantage over e + e − annihilations, where this s-channel process is highly suppressed. At c.m. energies √ s ee < ∼ 500 GeV, the effective cross-section for is at least a factor of four larger than any cross-section for Higgs production in e + e − annihilations. Moreover, the process e + e − → HZ requires considerably higher c.m. energies than γγ → H. Any theoretical model based on the gauge principle must evoke spontaneous symmetry breaking. In the minimal supersymmetric extension of the Standard Model (MSSM), for instance, spontaneous electroweak symmetry breaking results in five physical Higgs-boson states: two neutral scalar fields h 0 and H 0 , a pseudoscalar A 0 and two charged bosons H ± . In e + e − annihilations, the heavy neutral MSSM Higgs bosons can be created only by associated production (e + e − → H 0 A 0 ), whereas in γγ collisions they are produced as single resonances (γγ → H 0 , A 0 ) with masses up to 80% of the initial e − e − collider energy [11]. For example, if their masses are around 500 GeV, then H 0 and A 0 could be produced either in pairs in e + e − annihilations at √ s ee ≃ 1 TeV, or as single particles in γγ collisions at √ s ee ∼ 600 GeV.
The reaction γγ → H, which is related to H → γγ, proceeds through a 'loop diagram' and receives contributions from all charged particles that couple to the photon and the Higgs boson. Thus, the two-photon width Γ(H → γγ) is sensitive to the Higgs-top Yukawa coupling, as well as mass scales far beyond the energy of the γγ collision. Assuming that the branching ratio BR(H → bb) can be measured to an accuracy of about 2% in the process e + e − → HZ, the γγ partial width can be determined with a similar precision by measuring the cross-section Each of the decay modes H →bb, WW can be measured in photon-photon collisions with a precision comparable to that expected from analyses based on e + e − data (see, e.g., [12]).
High-energy photons can be produced by Compton-backscattering of laser light on electron beams. Both the energy spectrum and polarization of the backscattered photons depend strongly on the polarizations of the incident electrons and laser photons. The key advantage of using e − e − beams is that they can be polarized to a high degree, enabling one to tailor the photon energy distribution to one's needs. In a γγ collision, the possible helicities are 0 or 2. The Higgs boson is produced in the J z = 0 state, whereas the background processes γγ → bb, cc are suppressed for this helicity configuration. The circular polarization of the photon beams is therefore an important asset, for it can be used both to enhance the signal and suppress the background.
The CP properties of any neutral Higgs boson that may be produced at a photon collider can be directly determined by controlling the polarizations of Compton-scattered photons [13]. A CP-even Higgs boson couples to the combination e 1 · e 2 , whereas a CP-odd Higgs boson couples to (e 1 × e 2 ) · k γ , where e i are polarization vectors of colliding photons, φ is the angle between them, and k γ is the momentum vector of one of the Compton-scattered photons. The scalar (pseudoscalar) Higgs boson couples to linearly polarized photons with a maximum strength if the polarization vectors are parallel (perpendicular).
The general amplitude for a CP-mixed state to couple to two photons can be expressed as where E is the CP-even and O the CP-odd contribution to the amplitude. If we denote the helicities of the two photons by λ 1 and λ 2 , with λ 1 , λ 2 = ±1, then the above vector products read e 1 · e 2 = −(1 + λ 1 λ 2 )/2 and (e 1 ×e 2 ) z = iλ 1 (1 + λ 1 λ 2 )/2. As shown in [13], one can define three polarization asymmetries that yield an unambiguous measure of CP-mixing. Note that it is necessary to have both linearly and circularly polarized photons in order to measure those asymmetries. In e + e − annihilations, it is possible to discriminate between CP-even and CP-odd neutral Higgs bosons, but would be difficult to detect small CP-violating effects (which contribute only at the one-loop level) for a dominantly CP-even component (which contributes at the tree level in e + e − collisions) [14].
A study of single Higgs-boson production in γγ collisions via the hadronic content of the photon (resolved processes) was reported in [15]. Such contributions to γγ → H are non-negligible. Resolved photon production of the heavy MSSM Higgs bosons H 0 and A 0 would complement other measurements by probing particular regions of the SUSY parameter space [15].
To ascertain the physics potential of a γγ collider, one must take into account the fact that the photons are not monochromatic [16]. As already mentioned, both the energy spectrum and polarization of the backscattered photons depend strongly on the polarizations of the incident electrons and photons. A longitudinal electron-beam polarization of 90% and a 100% circular polarization of laser photons are customarily assumed. 4 Higgs-pair production in γγ and e + e − collisions It is well known that hadron colliders are not ideally suited for measuring the self-coupling of the Higgs boson if m H ≤ 140 GeV [17]. The potential of a future γγ/e + e − collider for determining the HHH coupling has therefore been closely examined (see [18] and [19]- [23]). The production of a pair of SM Higgs bosons in photon-photon collisions, γγ → HH (7) which is related to the Higgs-boson decay into two photons, is due to W-boson and top-quark box and triangle loop diagrams. The total cross-section for γγ → HH in polarized photon-photon collisions, calculated at the leading one-loop order [24] as a function of the γγ c.m. energy and for m H between 115 and 150 GeV, is given in [18]. The cross-section calculated for equal photon helicities, σ γγ → HH (J z = 0), rises sharply above the 2m H threshold for different values of m H , and has a peak value of about 0.4 fb at a γγ c.m. energy of 400 GeV. In contrast, the cross-section for opposite photon helicities, σ γγ → HH (J z = 2), rises more slowly with energy because a pair of Higgs bosons is produced in a state with orbital angular momentum of at least 2 (see Fig. 3). The cross-sections for equal photon helicities are of special interest, since only the J z = 0 amplitudes contain contributions with trilinear Higgs self-coupling. By adding to the SM Higgs potential V (Φ † Φ) a gauge-invariant dimension-6 operator (Φ † Φ) 3 , one introduces a gauge-invariant anomalous trilinear Higgs coupling δκ [24]. For the reaction γγ → HH, the only effect of such a coupling in the unitary gauge would be to replace the trilinear Higgs coupling of the SM, λ HHH , by an anomalous Higgs self-coupling λ = (1 + δκ)λ HHH . The dimensionless anomalous coupling δκ is normalized so that δκ = −1 exactly cancels the SM HHH coupling. The cross-sections σ γγ → HH for five values of δκ are shown in Fig. 3.
In an experiment to measure the trilinear Higgs self-coupling, the contribution from γγ → HH for opposite photon helicities represents an irreducible background. However, this background is suppressed if one chooses a γγ c.m. energy below about 320 GeV.
The Feynman diagrams for the process γγ → HH are shown in [24]. New physics beyond the SM introduces additional complexity into the subtle interplay between the Higgs 'pole amplitudes' and the top-quark and W-boson 'box diagrams': where λ SM is the trilinear Higgs self-coupling in the SM. From this expression we infer that the cross-section is a quadratic function of the coupling λ ≡ λ SM + δλ.
The trilinear self-coupling of the Higgs boson can also be measured either in the so-called double Higgs-strahlung process e + e − → HHZ (10) or in the W-fusion reaction The total cross-section for pair production of 120-GeV Higgs bosons in e + e − collisions, calculated for unpolarized beams, are shown in Fig. 4 for anomalous trilinear Higgs self-couplings δκ = 0 or −1. If the electron beam is 100% polarized, the double Higgs-strahlung cross-section will stay approximately the same, while the W-fusion cross-section will be twice as large. From the plots in Fig. 4 we infer that the SM double Higgs-strahlung cross-section exceeds 0. For m H = 120 GeV, and assuming a longitudinal electron-beam polarization of 90%, the maximum sensitivity to an anomalous trilinear Higgs self-coupling is achieved in the so-called double Higgs-strahlung process at a c.m. energy of about 500 GeV [18]. This is significantly higher than the optimal c.m. energy in γγ collisions. In the W-fusion process, a similar sensitivity is attained at c.m. energies well above 500 GeV.
Calculations show that the statistical sensitivity of σ γγ → HH to the Higgs self-coupling is maximal near the kinematic threshold for Higgs-pair production if m H ∼ 120 GeV, and is comparable with the sensitivities of σ e + e − → HHZ and σ e + e − → HHνν to this coupling for √ s ee ≤ 700 GeV, even if the integrated luminosity in γγ collisions is only one third of that in e + e − annihilations [18]. The overall acceptance should, in principle, be considerably larger in the process γγ → HH than in the reaction e + e − → HHZ due to the smaller final-state particle multiplicity.
Since the cross-section σ γγ → HH does not exceed 0.4 fb, it is essential to attain the highest possible luminosity, rather than energy, in order to measure the trilinear Higgs self-coupling. As shown in [18], appropriate angular and invariant-mass cuts and a reliable b-tagging algorithm are needed in order to suppress the dominant WW, ZZ and four-quark backgrounds well below the HH signal.
The results of detailed feasibility studies for measuring Higgs-pair production in γγ and e + e − collisions have been reported [25,26]. It has been shown that the optimum γγ collision energy is around 270 GeV for a 120-GeV Higgs boson, and that the main backrounds at this energy are the processes γγ → WW, ZZ and bbbb. The preliminary analysis described in [25] suggests that the process γγ → HH could be observed with a statistical significance of about 5σ, provided proper color-singlet clustering is used in jet reconstruction. The precision with which the trilinear Higgs self-coupling could be measured in the process e + e − → HHZ at √ s ee = 500 GeV and in the reaction e + e − → HHν eνe at √ s ee = 1 TeV is presented in [26].  Credit: R. Belusevic and J. Jikia [18].

5
The proposed facility A schematic layout of the proposed SLC-type e + e − /γγ facility is shown in Fig. 5. Damped and bunch-compressed electron and positron beams, accelerated by a single linear accelerator (linac), traverse two arcs of bending magnets in opposite directions and collide at an interaction point surrounded by a detector. The beams are then disposed of, and this machine cycle is repeated at a rate that depends on whether the linac is made of L-band or X-band accelerating structures. Using an optical free electron laser (FEL), high-energy photons for a γγ collider are created by Compton backscattering of FEL photons on electrons prior to their collision. With a crossing angle at the interaction point (IP), separate beam lines may be used to bring the disrupted beams to their respective dumps, thereby enabling post-IP diagnostics. It is also envisaged that a 'bypass line' for low-energy beams would be employed to accumulate data at the Z resonance in the process e + e − → Z. These runs could be used to regularly calibrate the detector, fine-tune the accelerator and measure its luminosity.
The proposed facility could be constructed in several stages, each with distinct physics objectives that require particular center-of-mass (c.m.) energies: For instance, the top-quark mass could be measured in the process e + e − → tt at the pairproduction threshold; one expects δm t ≈ 100 MeV ≈ 0.1δm t (LHC) [27]. The linac at the proposed SLC-type facility would consist either of (1) high-gradient X-band cavities developed for CLIC and a corresponding klystron-based power source (a two-beam scheme could be implemented at a later stage); or (2) ILC-type superconducting L-band cavities placed within cryogenic vessels and fed by multi-beam klystrons. The 11.4 GHz X-band rf technology was originally developed at SLAC and KEK. The choice of this technology is motivated by the cost benefits of having relatively low rf energy per pulse and high accelerating gradients. A comprehensive review of the status of X-band accelerator technology is given in [28]. Since then, significant advances have been made in pulsed HV and rf power generation, high gradient acceleration and wakefield suppression. The ultimate design of rf cavities will depend on the outcome of the ongoing effort to develop 100 MeV/m X-band structures for a CLIC-type linear collider.
As proposed in [23], a single X-band rf unit contains a modulator that drives a pair of 50 MW klystrons, each of which generates 1.6 µs rf pulses at 50 Hz. An rf compression system enhances the peak power of the klystrons by a factor of 3.75, and produces 245 ns pulses that match the accelerator structure requirements. The resulting 375 MW, 245 ns pulses feed seven 0.21m-long accelerator structures, producing a 85 (100) MV/m loaded (unloaded) gradient in each structure.
The current design for the International Linear Collider (ILC), based on the superconducting technology originally developed at DESY, uses L-band (1.3 GHz) superconducting niobium rf cavities that have average accelerating gradients of 31.5 MeV/m (see [29] and references therein). Nine cavities, each 1 m long, are mounted together in a string and assembled into a common low-temperature cryostat or cryomodule. Liquid helium is used to cool cavities to −271 • C.
An ILC-type main linac is composed of rf units, each of which is formed by three contiguous cryomodules containing 26 nine-cell cavities. Every unit has an rf source, which includes a pulse modulator, a 10 MW multi-beam klystron, and a waveguide system that distributes the power to the cavities. An ILC-type design offers some advantages over the X-band technology: • Wakefields are drastically reduced due to the large size of the rf cavities, which means that cavity alignment tolerances can be relaxed. This is crucial for an SLC-type facility, where both e + and e − bunches are alternately accelerated; • Superconducting rf cavities can be loaded using a long rf pulse (1.5 ms) from a source with low peak rf power; • 'Wall-plug to beam' power transfer efficiency is about twice that of X-band cavities; • The long rf pulse allows a long bunch train (∼ 1 ms), with many bunches (∼ 3000) and a relatively large bunch spacing (∼ 300 ns). A trajectory correction (feedback) system within the train can therefore be used to bring the beams into collision.
However, in contrast to a compact, high-gradient X-band machine, a collider based on the current ILC-type design would be characterized by (a) low accelerating gradients; (b) two large damping rings with a total length of at least six kilometers, and (c) a technologically challenging cryogenic system that requires a number of surface cryogenic plants.
An important feature of the proposed SLC-type facility is the possibility of using backscattered laser beams to produce high-energy γγ collisions [16]. In order to attain maximum luminosity at a γγ collider, every electron bunch in the accelerator should collide with a laser pulse of sufficient intensity for 63% of the electrons to undergo a Compton scattering. This requires a laser system with high average power, capable of producing pulses that would match the temporal spacing of electron bunches [23].
These requirements could be satisfied by an optical free electron laser (FEL) [30]. The radiation produced by an FEL has a variable wavelength, and is fully polarized either circularly or linearly depending on whether the undulator is helical or planar, respectively. The wavelength λ of FEL radiation is determined by λ ≈ λ u /2γ 2 , where γ ≡ E/m e c 2 is the Lorentz factor of the electron beam with energy E and λ u is the periodic length of the undulator. To produce photon pulses of required intensity, suitable high-intensity, low-emittance rf guns have to be developed [31].
Assuming that the mean number of Compton interactions of an electron in a laser pulse (the Compton conversion probability) is 1, the conversion coefficient k ≡ n γ /n e ≈ 1 − e −1 = 0.63, where n e is the number of electrons in a 'bunch' and n γ is the number of scattered photons. The luminosity of a gamma-gamma collider is then L γγ = (n γ /n e ) 2 L ee ≈ (0.63) 2 L ee (12) where L ee is the geometric luminosity at a conventional two-linac collider: In this expression, β x , β y are the horizontal and vertical beta functions, respectively, ε xn , ε yn are the normalized transverse beam emittances, N b is the number of bunches per rf pulse, f is the pulse repetition rate, √ s ee is the c.m. energy, and P beam = n e N b f √ s ee is the beam power. There are N b /2 electron or positron bunches in each arc of an SLC-type facility. If its repetition rate is twice that of a conventional two-linac collider, so that roughly the same wall-plug power is used, the two machines would have the same luminosity (see Eq. (13)).
The energy loss per turn due to synchrotron radiation (SR) in a storage ring is given by where C γ = 88.46 × 10 −6 m/GeV 3 , E [GeV] is the beam energy, ρ [m] is the effective bending radius, s [m] is the beam path length, and A ≡ 3C γ E 3 0 /2π. For E 0 = 250 GeV and ρ = 12 km, the expression on the left yields ∆E = 14.4 GeV per half turn; for E 0 = 350 GeV and the same radius, ∆E = 55.3 GeV per half turn. If there are no accelerating structures in the arcs, the linac energy must be increased, e.g., from E 0 = 300 GeV to E 0 ≈ 350 GeV in order to attain √ s ee = 600 GeV.
where γ is the Lorentz factor of the beam, C q ≈ 3.84 × 10 −13 m, and ρ [m] is the bending radius.
In contrast to ILC or CLIC, an SLC-type collider would have a single bunch compression system and a short beam transfer line connecting the damping rings with the entrance to the main linac (see Fig. 5). A 350-GeV superconducting L-band linac at the proposed facility may form, together with a 3-TeV energy booster, the injector chain for a proton collider in the FCC tunnel (e.g., the linac could replace the chain LINAC4 → PSB → PS → SPS at CERN).

Concluding remarks
It is proposed to place the arcs of an SLC-type facility inside the 100 km long tunnel of a Future Circular Collider (FCC). Electron and positron beams, accelerated in a single X-band or L-band linac, would traverse the arcs of bending magnets in opposite directions (see Fig. 5) and collide at c.m. energies considerably exceeding those attainable at circular e + e − colliders. Using an optical free-electron laser (FEL), the SLC-type facility could be converted into a γγ collider. Large savings in construction cost could be achieved if the crossing angle and the beam dump are exactly the same for the operation of the SLC-type facility in the e + e − and γγ collision modes.
The proposed e + e − /γγ collider could be built in several stages, each with distinct physics objectives that require particular c.m. energies (see Sections 2-5). The following unique features of the proposed facility are particularly noteworthy: • The maximum luminosity at a circular e + e − collider is severely constrained by beamstrahlung effects at high energies; also, it is very difficult to achieve a high degree of beam polarization [32]. This is not the case at an SLC-type facility, where luminosity is proportional to beam energy and the electron beam polarization can reach about 90%. The availability of polarized beams is essential for some important precision measurements in e + e − and γγ collisions [33].
• It is straightforward to convert an SLC-type facility into a high-luminosity γγ collider with highly polarized beams. This considerably increases its physics potential (see below).
• A 350-GeV superconducting L-band linac at the proposed facility may form, together with a 3-TeV energy booster, the injector chain for a 100-TeV proton collider in the FCC tunnel. The L-band linac could also be used to produce high-intensity neutrino, kaon and muon beams for fixed-target experiments, as well as X-ray FEL photons for applications in material science and medicine [34].
• If electron or positron bunches, accelerated by the L-band linac at the proposed facility, are brought into collision with the 50-TeV FCC proton beams, the whole accelerator complex could serve also as a source of deep-inelastic ep interactions [35]. Such interactions would yield valuable information on the quark-gluon content of the proton, which is crucial for precision measurements at the FCC hadron collider . The physics potential of an ep collider is discussed, e.g., in [36].
The rich set of final states in e + e − and γγ collisions at the proposed SLC-type facility would play an essential role in measuring the mass, spin, parity, two-photon width and trilinear selfcoupling of the SM Higgs boson, as well as its couplings to fermions and gauge bosons. Such measurements require c.m. energies considerably exceeding those attainable at circular e + e − colliders. For instance, one has to measure separately the couplings HWW, HHH and Htt at √ s ee > ∼ 500 GeV in order to determine the corresponding SM loop contributions to the effective HZZ coupling (see Sections 2-5 and, e.g., [37]).
For some processes within and beyond the SM, the required c.m. energy is considerably lower in γγ collisions than in e + e − or proton-proton interactions. For example, the heavy neutral MSSM Higgs bosons can be created in e + e − annihilations only by associated production (e + e − → H 0 A 0 ), whereas in γγ collisions they are produced as single resonances (γγ → H 0 , A 0 ) with masses up to 80% of the initial e − e − collider energy.
Both the energy spectrum and polarization of the backscattered photons at a γγ collider depend strongly on the polarizations of the incident electrons and laser photons. The circular polarization of the photon beams is an important asset, for it can be used both to enhance the signal and suppress the background. The CP properties of any neutral Higgs boson produced at a photon collider can be directly determined by controlling the polarizations of Compton-scattered photons.