Abstract
Single photons are of paramount importance to future quantum technologies, including quantum communication and computation. Nonlinear photonic devices using parametric processes offer a straightforward route to generating photons, however additional nonlinear processes may come into play and interfere with these sources. Here we analyse spontaneous fourwave mixing (SFWM) sources in the presence of multiphoton processes. We conduct experiments in silicon and gallium indium phosphide photonic crystal waveguides which display inherently different nonlinear absorption processes, namely twophoton (TPA) and threephoton absorption (ThPA), respectively. We develop a novel model capturing these diverse effects which is in excellent quantitative agreement with measurements of brightness, coincidencetoaccidental ratio (CAR) and secondorder correlation function g^{(2)}(0), showing that TPA imposes an intrinsic limit on heralded single photon sources. We build on these observations to devise a new metric, the quantum utility (QMU), enabling further optimisation of single photon sources.
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Introduction
Photons are a key building block for future quantum technologies and are the most suitable choice for linking distant quantum systems^{1}. Deterministic single photon sources based on quantum dots^{2} and defects in diamond^{3} are being heavily investigated, however they are currently limited due to the inherent randomness of emission direction, large bulk optical collection setups and most often the use of cryogenic temperatures, all of which make this technology challenging to scale up. The generation of photons through probabilistic processes in bulk nonlinear materials has been a workhorse for quantum information experiments^{4,5,6,7,8}. In recent years, integrated waveguide devices have emerged as an attractive platform for scalable quantum technologies^{7,8,9,10,11,12,13,14,15,16,17,18,19}. These chipscale platforms are typically made of glasses, such as silica and chalcogenide, or semiconductors such as silicon (Si) and gallium indium phosphide (GaInP). In contrast to earlier freespace investigations, one must consider additional effects induced by the media and their role in the generation and collection of photons. In amorphous materials, spontaneous Raman scattered photons act as a noise source, dramatically impacting the desired quantum statistics^{10,19,20}. In crystalline semiconductor materials multiphoton absorption and accompanying free carrier effects are present at larger intensities. While the roles of multiphoton effects in the classical regime are reasonably well known^{21,22,23,24,25,26,27,28,29}, quantum pair generation processes in these materials have only recently been investigated^{11,12,13,14,15,16,17,18}. Though these initial observations noted that nonlinear absorption affected the experiments, at present the nuanced roles of the multiphoton processes in the quantum regime is unclear.
In this paper we analyse the interaction of probabilistic photon generation with multiphoton processes in both the generation and collection of single photons for the first time. We carry out experiments in Si^{16,17} and GaInP^{18} semiconductor waveguides which display inherently different nonlinear absorption processes, namely twophoton (TPA) and threephoton absorption (ThPA), respectively. We develop a novel model capturing these effects, including slowlight enhancements in the photonic crystal periodic media^{16,17,18,21,22,23,24,25,26}. The series of measurements of brightness, coincidencetoaccidental ratio (CAR) and secondorder correlation function g^{(2)}(0) are in excellent quantitative agreement with our theoretical model, demonstrating this framework is suitable for predicting photon generation in the presence of strong nonlinear effects. We show that TPA imposes an intrinsic limit on heralded single photon generation even in the single photon pair regime. We finally devise a new metric, the quantum utility or QMU, that unites several key parameters of single photon devices and show an example of its use to improve our current devices. This metric should facilitate the development of optimised multiplexed and integrated photon sources, thereby opening new routes to scalable quantum computation and simulation with large numbers of photonic qubits.
Figure 1 illustrates the various nonlinear processes considered. Photons from a pulsed laser are injected to the thirdorder χ^{(3)} nonlinear device, where a number of processes can occur. The primary process for the generation of photons is spontaneous fourwave mixing (SFWM) where two pump photons are annihilated to generate entangled signal and idler photons at higher and lower energy, respectively. The nonlinear absorption processes include TPA, the markedly weaker ThPA, and any related free carrier absorption (FCA) induced by electrons generated from these processes. We include these losses to the pump photons propagating through the nonlinear medium, as well as through crossTPA (XTPA) between a pump photon and a signal or idler photon. Though XTPA between the generated signal and idler photons is also possible, this is a weak effect due to the small intensities of single photons and is neglected here. In the experiments we found ThPA and crossThPA play negligible roles in the quantum regime. Consequently, we focus the discussion on TPA, XTPA, and FCA.
Results
Heralded single photon generation with multiphoton absorption
The novelty of our approach is the incorporation of nonlinear absorption processes in four major aspects of SFWM photon pair generation and collection. The generation terms are described by the interaction of multiphoton absorption with the strong pump beam. In this regard, TPA impacts both (i) the nonlinear phase shift Φ (radians), as well as (ii) the phase matching of the parametric process. Once generated, multiphoton absorption also affects (iii) the absorption of the signal or idler single photons with the copropagating pump beam via XTPA and (iv) absorption of single photons by freecarriers generated by the pump (FCA).
First, we consider the impact of TPA on the probability of generating a pair of photons per laser pulse, μ. In the case of SFWM, this probability scales as μ ~ Φ^{2}Θ^{2} with the nonlinear phase shift Φ and phase matching terms Θ (see Supplementary Information). In the presence of TPA, Φ scales logarithmically with power^{28}
where γ = k_{o}n_{2}/A_{eff} is the nonlinear parameter, Kerr coefficient n_{2}, effective area A_{eff}, wave number k_{0}, α_{2} the TPA coefficient, I_{0} = P_{o}/A_{eff} the pump intensity with peak power P_{0}, L_{eff} = 1 − exp(−αL)/(α) the effective device length with scattering loss α, and S = (n_{g}/n_{0}) the slowdown factor in the photonic crystal waveguide (PhCW)^{22,24,30}. Similar scaling occurs for coupledcavity waveguides^{15,31}. In the experiments we control Φ by varying the input laser power. While earlier work suggests the role of TPA in reducing coincidence counts in the SFWM process^{11,12,13,14,15,16,17,18}, here we describe the various roles of nonlinear absorption and quantitatively include these effects in our photon pair model. While this description of Φ is pertinent to Si, we note that a linear definition of Φ = γS^{2}P_{0}L_{eff} is appropriate for GaInP at the power levels used in these experiments. Second, as SFWM is a parametric process one must also consider the phase matching conditions. In particular, Θ is a function of Φ (see Supplementary Information).
Further to these two mechanisms where TPA influences the pump during pair generation, multiphoton absorption also strongly affects the generated single photons by introducing two loss channels in the collection. The third impact of multiphoton absorption is a collection loss due to absorption of single photons through XTPA of the signal or idler single photons with the copropagating pump beam. For two copolarised beams, this effect is described by
where η_{XTPA} ≤ 1 is the collection efficiency per photon. The fourth impact of multiphoton absorption is the generation of free carriers during pump propagation via TPA. FCA of single photons is described by
where σ is the absorption cross section, N_{c} is the carrier density and L_{eff}(2α) = 1 − exp(−2αL)/(2α)^{21,28}. Equivalent expressions exist for ThPA, though we exclude these here due to the fact that they are negligible at intensity values required for heralded single photons from SFWM. This is the first time the role of multiphoton absorption, in particular TPA, XTPA, and FCA, have been quantitatively analysed in photon pair generation and collection. We note equivalent expressions could be derived for microcavities, where the nonlinear enhancement arises from the ratio of quality factor (Q) to mode volume (V)^{32}, and other slowlight structures such as coupledresonator optical waveguides (CROW)^{15,33}. Single photon sources based on downconversion in χ^{(2)} media such as AlGaAs waveguides would also have to consider these effects^{34,35}. Notably, experimental evidence indicates the material α_{2} parameter in down conversion experiments can be much larger than the present case due to the extreme nondegeneracy of the photons^{29} in contrast to our nearly degenerate case.
Experiments and modeling of SFWM pair generation in photonic crystal waveguides: linear and TPA regimes
We performed a number of experiments on photonic crystal waveguides fabricated in two different nonlinear semiconductor materials, namely Si and GaInP, to examine the heralded photon generation in the presence of nonlinear absorption and compare them to theoretical predictions (see Methods section for device and experimental details). At large intensities these materials exhibit two and threephoton absorption, respectively, for the photon energies (0.8 eV) in our experiments.
To confirm these observations we create a model for the generation, filtering and detection system, shown in Fig. 2, which we treat in a similar way to Bussières et al.^{36}. For the generation term, we define p_{i} as a thermal distribution dependent on μ, the number of pairs per pulse (including our TPA and slowlight modifications). This distribution is appropriate when the filtering matches the pump pulse bandwidth^{37}. For the photon pair collection, we create a vector describing the state of the detector system indicating the probability of each detector switching from the unclicked state to the clicked state (see Methods and Supplementary Information). We construct accompanying matrices describing the (i) detector dark counts M_{D} and (ii) loss mechanisms of generated photons in the system M_{η} (see Methods section). The M_{η} matrix describes the photon collection efficiencies , as well as intrinsic losses of single photons due to propagation η_{α} = exp(−αL) and our newly derived nonlinear loss terms η_{NL} = η_{XTPA}η_{FCA}
where the subscripts S, I correspond to the signal and idler channels, respectively. These matrices act on an original vector set to an initial unclicked state and are populated with a thermal distribution of photons related to μ. We account for the probability of generating multiple pairs per pulse in the SFWM process through terms proportional to μ^{n}, where n is the number of generated photon pairs. The final output vector provides the total probability for all detector states and coincidence terms.
Figure 3(a) shows the experimentally measured coincidence counts versus Φ for Si (at a groupvelocity dispersion (GVD) of β_{2}. β_{2} = −0.9 ps^{2}/mm). The modelled results are in excellent agreement with the experimental data points in terms of both the SFWM photon coincidence counts (upper curves) and the accidental coincidence counts arising from detector dark counts, multipair emission and any residual leaked pump (lower curves). The black lines are theoretical curves with numerically suppressed TPA (and therefore FCA) showing a significant increase in both coincidences and accidentals. Of particular interest is the flattening to a maximum count of less than fivepersecond for the Si device due to both the restricted Φ in the generation, as well as XTPA and FCA of the generated pairs in the collection.
Using the coincidence count data, we calculate the coincidencetoaccidental ratio (CAR), a metric analogous to a signaltonoise ratio in a classical system. Fig. 3(b) shows the experimental data along with the modelled values once again demonstrating excellent agreement. The black curve in Fig. 3(b) shows a numerical suppression of TPA only slightly reducing the maximum CAR value, despite the strongly suppressed coincidence counts seen in Fig. 3(a). Comparing the strongly modulated coincidence counts in Fig. 3(a) with the relatively unaffected CAR in Fig. 3(b), it is clear that one must look beyond CAR as a simple metric for probabilistic photon sources.
We calculated the coincidence counts and CAR as a function of both group velocity dispersion (GVD) and Φ, including slowlight effects in the PhCW^{21,22,24}. Figures 3(c) and (d) show numerically computed contour plots of the coincidence counts and car for Si. The experimental device GVDlength product is indicated by the dashed white line through the plot (β_{2}L = −0.18 ps^{2}). The experimental wavelength is determined by the frequency spacing of our arrayed waveguide grating (AWG) filter. We observe in Figs. 3(c) and (d) that both GVD and Φ determine the best operating point, a fact that must be taken into consideration when designing and fabricating photon pair sources based on SFWM. The tilt of the coincidence contours towards anomalous (negative) GVD is required to balance the nonlinear (positive) contribution to the phase matching. We note the nonlinear contribution dominates in these chipscale devices in contrast to the linear dispersion contribution that is more significant for fibrebased sources^{20,38,39,40}. In the case of Si, TPA additionally saturates Φ, as noted previously, causing an adjustment to the nonlinear phase matching contribution for photonpair generation.
We next performed identical measurements in a GaInP PhCW, a material free from TPA in the telecommunications band (E_{g} = 1.9 eV)^{21,23,26}. Figure 3(e) shows the experimentally measured coincidence counts versus Φ for GaInP (β_{2} = −0.13 ps^{2}/mm). Note the xscale (Φ) is smaller for ease of comparison to the coincidence counts (yscale) with the Si case. In contrast to the rolloff in the TPAlimited material, GaInP exhibits no deviation from the expected quadratic photon pair coincidence rate. Importantly, the ThPA intensity threshold is not reached at the power levels required to generate photon pairs. Essentially GaInP behaves as a linear material in the regimes of interest. Figure 3(f) indicates the measured CAR for the GaInP experiments. The maximum CAR for this device is smaller than Si due to increased linear propagation loss in the longer device of 1.5 mm versus the 0.2 mm for Si. Contour plots of the coincidences and CAR are shown in Fig. 3(g) and (h) for GaInP, with white dashed lines once again indicating the experimental GVDlength product (β_{2}L = −0.20 ps^{2}). Notice that despite very different behaviour in coincidence counts, the CAR plots for Si  Fig. 3(d) and GaInP  Fig. 3(h) behave comparatively at large Φ due to multipair generation.
Secondorder correlation function measurements
The secondorder correlation function, or g^{(2)}(0) is another important metric for single photon sources. The g^{(2)}(0) is an indicator of how well the source output compares to a single photon^{18,36,41}. A g^{(2)}(0) of 0 corresponds to an ideal single photon source while a standard coherent Poissonian light source exhibits a g^{(2)}(0) value of 1. For our threedetector heralded measurement this is described by
where Π_{j}_{H} are the conditional probabilities that the j^{th} detector is triggered when the herald detector H is also triggered (see Supplementary Information). We desire large Π_{A}_{H} or Π_{B}_{H} which indicate true single photon pairs while simultaneously minimizing Π_{AB}_{H} (triples  multiple photons)^{36,41}. To measure this quantity one detects a first photon (the signal) heralding the arrival of a second photon (the idler) with this latter photon passing through a 50:50 coupler and sent to one of two detectors. True single photons will only trigger one of these two detectors. If there is a coincident count across these two detectors the g^{(2)}(0) rises above the ideal value of zero indicating more than a single photon is present.
Figure 4(a) shows our g^{(2)}(x) measurements for the two platforms, where x corresponds to the integer number of delayed pulse periods of one of the heralded photons with respect to the other. True heralded single photon operation only occurs in the g^{(2)}(0) window, achieving minimum g^{(2)}(0) values of 0.09 for Si and 0.06 for GaInP. When x is nonzero, the heralding of the output photon is lost, and the statistics revert to a coherent Poissonian source with g^{(2)}(x) values of 1, as expected.
The evolution of the g^{(2)}(0) parameter as a function of Φ is shown in Figs. 4(b) and (c) for Si and GaInP, respectively. To model g^{(2)}(0), we extend our previous twophoton formulation to accommodate three detectors. The chief sources increasing g^{(2)}(0) include dark counts at small Φ and multipair generation at larger Φ. In both cases the extended g^{(2)}(0) model is once again in solid agreement with the experimental data. The minimum of the g^{(2)}(0) function corresponds to the onset of the multiple pairsperpulse (i > 1) (see Supplementary Information).
The present limit to these values is detector dark counts, not the devices themselves. In particular, for the g^{(2)}(0) experiments, we required a larger detection efficiency of η_{D} = 10% (compared to 7.5% for the CAR experiments) in order to obtain significant counting statistics for the threephoton g^{(2)}(0) measurements. A unique aspect of our model is the ability to numerically extract the g^{(2)}(0) value from our low dark count experimental CAR data. The black dashed lines in Figs. 4(b) and (c) show the extrapolated results reveal a striking g^{(2)}(0) of 0.013 for GaInP and less than 0.007 in the case of Si, a near order of magnitude improvement over our prior record for PhCW devices^{18}. We expect near ideal singlephoton operation, g^{(2)}(0) → 0, in our devices with ultralow dark count detectors such as superconducting detectors^{42,43}. The GaInP is slightly higher due to higher propagation loss in the longer device.
Conversely, we extrapolate a CAR from our experimental g^{(2)}(0), shown as the red/blue dashed lines in Figs. 4(b) and (c). We observe the numerically extrapolated CAR is below the level achieved in the experimental CAR measurements, as expected from the higher dark count rate at η_{D} = 10%. An interesting feature of the overlaid g^{(2)}(0) and CAR plots is the noticeable correspondence between the minima in the g^{(2)}(0) and the maximum of the CAR. This feature is due to multipair generation at large Φ acting as the dominant noise source in these metrics. The g^{(2)}(0) rises above a value of 0.5 for larger Φ as expected (see Supplementary Information).
Implications of TPA and XTPA on heralded single photons
We now look more closely into the role of the multiphoton losses in heralded single photon sources and derive some general conclusions about TPAlimited processes. We describe the photon generation, which affects the pump beam phase shift Φ through TPA and the free carrier population N_{c}, detailed in the Supplementary Information. Here we focus on XTPA in the collection of single photons and coincidence counts as it has a more pronounced impact than TPA on pair generation. Recall the collection losses given by Eqn. 4 are per photon channel and thus coincidence counts are proportional to the intrinsic collection losses as: . Figure 5(a) shows the various collection efficiencies squared (proportional to coincidences) versus Φ. We indicate the experimental region in the plot (Φ < 0.8 radians  black line), as well as the single photon pair regime shown as the shaded area. The single photon pair region was determined by setting i = 1 in the model and is consistent for both Si and GaInP. Immediately one notices XTPA is the dominant source of loss in the system, quickly decreasing from 100% even in the single photon pair regime.
The implications of this result are important for single photon sources exhibiting TPA. In particular, heralded single photon sources based on TPAlimited materials will require additional multiplexing, and therefore waveguides and footprint, to achieve the same efficiency compared to linear materials^{44,45}. FCA also sets in and further reduces coincidence counts in the single pair regime and plays a larger role with increasing Φ. Even at the maximum Φ, the estimated contributions of XThPA is <0.2 dB, nearly an order of magnitude smaller than XTPA and FCAinduced pair loss at the same Φ.
Finally, we consider materials with improved nonlinear figures of merit FOM_{NL} = n_{2}/(α_{2}λ) to discern whether TPA is truly an ultimate limit to photon pair generation. Fig. 5(b) shows η^{2} for various values of FOM_{NL}. Silicon (FOM_{NL} = 0.4) is indicated as the solid line, with hypothetical values of fourfold FOM_{NL} = 1 and tenfold FOM_{NL} = 4 lower α_{2} values suggesting drastic improvements. Though XTPA would be diminished in these materials, as η < 1, it is an impairment one must always consider when present. In addition to our experimental demonstrations in GaInP in this work^{21,23,26}, other wide bandgap materials such as AlGaAs^{27,46} and SiN^{47,48} are promising candidates for future single photon experiments. The advantages of a TPAfree material, even at the single photon level, will certainly be required for efficient photon generation.
Optimisation of photon sources: the quantum utility
It is clear from this study that developing the ideal photon source requires the optimisation of the output statistics across a number of metrics. For probabilistic photon sources, these include the achievable coincidence count rate, CAR and g^{(2)}(0), which are difficult to optimise simultaneously in a practical environment. While CAR and g^{(2)}(0) are well established measures of probabilistic photon sources, at present no single parameter encapsulates the performance of these devices. With this in mind we have developed a new metric for single photon sources which we term the quantum utility, or QMU, defined as
where μ′ is the single photon collection efficiency after any intrinsic device losses.
For a single probabilistic source, μ′ = μη^{2}, with η^{2} due to propagation and nonlinear losses as defined above, and g^{(2)}(0) is a heralded g^{(2)}(0) measurement. Note that the QMU is a positive value. In the absence of dark counts and noise photons, CAR scales as 1/μ, thereby making the QMU reach a value of one for a single ideal probabilistic photon source. Under these conditions, the CAR and g^{(2)}(0) would yield identical values, even with TPA. The experimental results, however, clearly indicate TPA, XTPA, and FCA reduce the number of coincidence counts as shown in Fig. 3, highlighting the importance of μ′ as an indicator of useful photon pairs. Note that μ′ excludes detector dark counts and any extrinsic losses. Moreover, this metric can be employed for systems without nonlinear loss by setting η_{NL} = 1 or slowlight by setting S = 1. Importantly, once the measurements are verified with a model, one can remove systemspecific effects such as collection or detector efficiencies and dark counts to extract an intrinsic CAR or g^{(2)}(0). Figure 6 shows the experimental points and modelled (solid line) values for the QMU of our devices. We see that the fabricated Si PhCW has a larger maximum QMU of ~0.22. We note that few other papers measure these three quantities in the same experimental setup, and it is consequently difficult to derive a QMU from the literature at present.
Building on our observations, we use the model to make a fair comparison of the Si and GaInP devices by assuming devices of the same length of 200 μm, same effective nonlinearities γ, matched group index n_{g} = 37 and coupling loss, all of which are experimentally achievable. We also consider operation at a more favourable phase matching condition than in our experiments by numerically setting the dispersion to β_{2} = −0.1 ps^{2}/mm (β_{2}L = −0.02 ps^{2}). Figure 6 indicates the numerically extrapolated QMU under these more favourable conditions shown as dashed lines. GaInP reaches a larger maximum QMU of 0.3 compared to the maximum of Si, which reaches a value of 0.25. In addition, the GaInP QMU is higher than Si for all values of the nonlinear phase shift Φ. This implies that GaInP will emit a greater number of coincident photons at a given CAR and g^{(2)}(0) over all coupled powers as compared to silicon. Separate plots of the individual μ′, CAR, and g^{(2)}(0) curves for the comparison case are in the Supplementary Information. At the maximum QMU for GaInP we expect a 5fold increase in the coincidence counts whilst maintaining a CAR of 30, meaning a fourphoton experiment such as quantum interference or an integrated quantum gate could be carried out in a matter of hours rather than days. With the QMU parameter we now have a succinct metric to compare and optimise singlephoton sources.
We close with commentary on the broader applicability of the QMU to various single photon sources. As we noted earlier, microcavity^{32,49}, χ^{(2)} waveguide devices^{34,35} would need to also consider appropriate definitions of the generation term μ′ and the nonlinear loss term η_{XTPA}. It is also possible to multiplex these single spontaneous heralded sources to create a pseudodeterministic single photon source^{44,45}. Single photon heralded sources composed of multiplexed probabilistic sources is an area of active research with integrated spatial multiplexing only demonstrated this year^{50} while temporal multiplexing currently remains undemonstrated^{51}. For a multiplexed heralded source, where the multipair noise is decoupled from the heralded photon rate, a QMU > 1 is possible and is indeed desirable. Concretely, one can operate at the same CAR across a series of multiplexed sources whilst increasing the single photon rate μ′, thereby exceeding the multipair limit of a single probabilistic source.
Discussion
We have described the interaction of probabilistic photon generation with multiphoton processes in both the generation and collection of single photons for the first time. We measured the CAR and g^{(2)}(0) of photon pairs generated from spontaneous fourwave mixing in two representative materials exhibiting twophoton absorption (Si) and threephoton absorption (GaInP), respectively. We developed a model to describe photonpair generation in highly nonlinear semiconductors incorporating these multiphoton absorption effects and associated freecarriers. The model accurately predicts output photon statistics including source brightness, coincidencetoaccidental ratio and secondorder correlation function for heralded photons. Using this model, we showed that TPA imposes an intrinsic limit on heralded single photon generation even in the single photon pair regime for different nonlinear figures of merit. Finally, we formulated a new parameter based on these simple metrics which allows us to optimise photon source parameters for future quantum information science experiments and technology. The development of these sources will be integral to increasing the complexity of quantum photonic experiments.
Methods
Basic formulation of the model
For a twophoton measurement system, such as that used to measure coincidence counts and CAR, we begin by constructing a vector which describes the joint state of the two detectors , for the signal and idler detectors S and I, where the bar corresponds to no detection. We initialise this vector in the unclicked state such that P_{0} = (1, 0, 0, 0) and then act upon this with matrices describing the detector dark counts, M_{D}, and system losses, M_{η}, which have size 2^{n} × 2^{n}, where n is the number of detectors for a number of photon pairs generated, i, such that
The probability distribution of photons p_{i} depends on the number of pairs generated per pulse, μ, from a thermal source such that
with the nonlinear absorption affecting μ as noted in the main text. Nonlinear losses η_{XTPA}, η_{FCA} are included as extra terms in M_{η}, however could equally be included as separate matrices. By analysing the output vector P on a per pulse basis we are able to extract the coincidences and singles counts, allowing a full calculation of the other metrics for analysing photon sources including the CAR. This method can be extended to three detectors for g^{(2)}(0) correlation function calculations, as described in the Supplementary Information.
Device specifications
The silicon PhCW device is fabricated from a silicon on insulator wafer with a 220 nm silicon membrane layer on 2 μm of silica using electron beam lithography and reactive ion etching. Further fabrication details are available in Ref. (22). The PhCW is made by creating a triangular lattice of holes (lattice parameter of a = 404 nm) with a row missing in the Γ − K direction with the silicon membrane suspended in air. The waveguide is 196 μm long with inverse tapers for improved coupling and polymer waveguides for mode matching to the lensed fibres. The two rows of holes (r = 0.285 a) adjacent to the waveguide are laterally shifted 50 nm outwards to engineer the dispersion^{52} such that the group index is 30 and is flat to within 10% across the SFWM bandwidth used and centred at a wavelength of 1540.6 nm. The effective nonlinearity γ_{eff} = γS^{2} = 5500 W^{−1}m^{−1} includes the slow light effect with a linear propagation loss of 65 dB.cm^{−1}, and α_{2} = 1 cm.GW^{−1} as determined by prior measurements^{22,53}. The dispersion was measured by Fourier transform spectral interferometry^{54}.
The GaInP device is a 1.5 mm long selfstanding membrane of 190 nm thickness with a lattice period a = 470 nm and radius r = 0.22 a. We incorporate inverse tapers to allow efficient mode conversion. Dispersion engineering is achieved through shifting the rows adjacent to the waveguide in opposite directions along the waveguide^{55}, achieving a group index of 20 in the slow light region with the pump centred at 1542.5 nm. The input facet of the GaInP was damaged and limited the amount of achievable phase shift. Coupling is estimated as 9.5 dB in/2.5 dB out. The effective nonlinearity in this device is γ_{eff} of 2300 W^{−1}m^{−1}, slightly lower than the silicon device, as extracted in our earlier work^{30,55,56} with a measured linear propagation loss of 30 dB.cm^{−1} and dispersion determined by optical frequency domain interferometry^{57}.
Experimental setup
A wavelength tunable CBand fibre laser provides 10 ps pulses at a repetition rate of 50 MHz which are passed through an isolator to protect the laser. Any residual pump cavity photons are removed by a WDM and any spontaneous Raman scattered photons from the silica fibers are removed with a tunable bandpass filter. The input power is monitored using a power meter. The input pulses are optimised for TE polarization using a polarization controller and coupled to the PhCW under test using 2 μm spot size lensed fibres. Signal and idler photons generated in the PhCW through SFWM are then separated using an arrayed waveguide grating which provides 40 dB of isolation from the pump. Further pump rejection is provided by tunable bandpass filters. We select AWG channels 600 GHz from the pump channel. The photons are then detected using InGaAs avalanche photodiode detectors (ID Quantique ID210) synchronized to the laser repetition rate and set to a detection efficiency of 7.5% resulting in dark counts of 1 × 10^{−6} and 2 × 10^{−6} per detection gate in the signal and idler detectors respectively. Coincidence counts are measured using a time interval analyser (TIA). For the g^{(2)}(x) correlation function measurements a 50:50 fiber coupler is added to the idler arm with the outputs connected directly to two InGaAs APDs (ID Quantique ID201) with efficiencies of 10% and dark count levels of 5 × 10^{−4} per detection gate. The efficiency of the detector in the heralding signal photon arm is increased to 10% to increase the 3fold coincidence rate and reduce measurement errors. This results in a marked increase to the dark counts in the heralding detector to 4 × 10^{−6} per detection gate.
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Acknowledgements
The authors thank Alex Judge for discussions on the CAR model as well as Luke Helt and Mike Steel for comments on the manuscript. This work was supported in part by the Centre of Excellence (CUDOS, project number CE110001018), Laureate Fellowship (FL120100029) and Discovery Early Career Researcher Award (DE120102069, DE130101148, and DE120100226) programs of the Australian Research Council (ARC), EPSRC UK Silicon Photonics (Grant reference EP/F001428/1), EU FP7 GOSPEL project (grant no. 219299), and EU FP7 COPERNICUS (grant no. 249012).
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A.C., C.H. and M.C. performed the measurements on the setup developed by M.C., C.X. and A.C. C.H. and A.C. performed the data analysis and modeling. C.H. derived the nonlinear analytic expressions and numerical simulations. S.C., G.L., and I.R. prepared the samples and nanofabrication. B.E., A.D.R., and T.K. supervised the project. C.H. and A.C. wrote the manuscript. All authors confirm the advances described in the paper.
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Husko, C., Clark, A., Collins, M. et al. Multiphoton absorption limits to heralded single photon sources. Sci Rep 3, 3087 (2013). https://doi.org/10.1038/srep03087
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DOI: https://doi.org/10.1038/srep03087
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