An all-silicon single-photon source by unconventional photon blockade
The lack of suitable quantum emitters in silicon and silicon-based materials has prevented the realization of room temperature, compact, stable, and integrated sources of single photons in a scalable on-chip architecture, so far. Current approaches rely on exploiting the enhanced optical nonlinearity of silicon through light confinement or slow-light propagation, and are based on parametric processes that typically require substantial input energy and spatial footprint to reach a reasonable output yield. Here we propose an alternative all-silicon device that employs a different paradigm, namely the interplay between quantum interference and the third-order intrinsic nonlinearity in a system of two coupled optical cavities. This unconventional photon blockade allows to produce antibunched radiation at extremely low input powers. We demonstrate a reliable protocol to operate this mechanism under pulsed optical excitation, as required for device applications, thus implementing a true single-photon source. We finally propose a state-of-art implementation in a standard silicon-based photonic crystal integrated circuit that outperforms existing parametric devices either in input power or footprint area.
The last decade has witnessed a tremendous progress in silicon-on-insulator (SOI) technology for applications in photonic integrated computing and data processing Streshinsky2013 (). In parallel, integrated photonic circuits have become increasingly appealing to realize key tasks in quantum information and communication, thanks to their natural interfacing with long distance communication networks working in telecommunication band ( m wavelengths). Clearly, the combination of these two paradigms will likely allow to realize complex quantum operations on-chip that are far beyond what may be envisaged with table-top experiments, with significant and large scale impact on efficient and secure data processing and transmission OBrien2013 (). Within this context, the generation of single photons plays a central role for the development of on-chip quantum photonic technologies OBrien2009 (). In particular, the recent advances in silicon-based quantum photonics Politi2008 (); Politi2009 (); Spring2013a (); Crespi2013 () would strongly benefit from integrated single-photon sources on the same operating chip.
Single-photon sources on-demand can be realized with artificial two-level emitters, such as semiconductor quantum dots Michler2000 (); Pelton2002 (), which have increasingly improved their radiative efficiency over the last few years Claudon2010 (); Reimer2012 (); He2013 (); Ates2013 (). However, these single photon sources are typically based on III-V semiconductors, they work most efficiently at cryogenic temperatures, and integration with silicon-based nanophotonic circuits working in the telecommunication band Streshinsky2013 () remains challenging. As a possible alternative, integrated single-photon sources in silicon-on-insulator (SOI) photonic circuits have been shown Davanco2012 (); Spring2013b (); Thompson2013 (), based on enhanced four-wave mixing induced by the silicon susceptibility and non-deterministic heralding. Even if the efficiency of such integrated sources can be improved by spatial multiplexing Collins2013 (), compactness and scalability remain open issues.
An alternative route to single-photon generation relies on the photon blockade mechanism Werner1999 (), where a strong third-order nonlinearity in an optical resonator enables a shift of the resonant frequency by more than its linewidth when a single photon is already present. As a consequence, the device can absorb a photon only after the previous one has been emitted. However, this mechanism however requires a stronger optical nonlinearity than what is achieved in state-of-the-art SOI devices Ferretti2012 ().
Here, we build on the mechanism called unconventional photon blockade (UBP), recently advocated as a promising paradigm for single-photon generation Liew2010 (); Bamba2011 (); Ferretti2013 (). The UPB mechanism relies on quantum interference, and is therefore highly sensitive to an optical nonlinearity of small magnitude. At difference with the conventional blockade, it has been shown that UPB can also occur when the nonlinear frequency shift per photon is much smaller than the cavity linewidth, which is usually the case also in silicon photonic crystal nanocavities Lai2014 (); Minkov2014 (); Dharanipathy2014 (). So far, such theoretical mechanism was only shown to work under continuous-wave (cw) excitation, which severely limits the usefulness of the proposed antibunched radiation as an actual single-photon source Bamba2011 (); Ferretti2013 (). In the present paper we go beyond previous works on UPB by demonstrating a reliable protocol that allows to operate any such system under pulsed excitation. In fact, this can be technically achieved by a combination of excitation pulse tailoring and post-selective temporal filtering of the output stream to purify the statistics of the emitted radiation, similarly to what has been already demonstrated for quantum dot-based single photon sources Ates2013 (). The latter achievement allows to overcome a previously believed limitation, and provides a scheme to devise a true single photon source out of a generator of antibunched radiation. The efficiency of such a single photon source in realistic devices is analyzed in detail, which is shown to outperform the best heralded sources demonstrated so far in key figures of merit, especially operation power and spatial footprint.
Following Refs. Liew2010, ; Bamba2011, , we consider UPB in a system of two tunnel-coupled cavities, i.e. a photonic molecule, as sketched in Fig. 1a. The quantum model of UPB has been thoroughly characterized Ferretti2013 (), and it is briefly summarized in the Methods section. The relevant physical parameters are the tunnel coupling rate between the two cavities (), the driving rate on the first cavity (), the driving frequency (), the effective photon-photon interaction energy in each cavity (, ), which originates from the intrinsic material Ferretti2012 (), and the cavities loss rates . Detrimental pure-dephasing processes are known to be negligible if the overall dephasing rate is much smaller than Ferretti2013 (). For a photonic crystal cavity in silicon, this condition is largely fulfilled Flayac2014 (). Finally, the model can be generalized to include input and output quantum channels Flayac2013 (). We will assume , and in the following, without loss of generality.
A scheme of the lowest 6 levels on the basis of photon-number states, , is given in Fig. 1b. The different excitation pathways leading from the initial ground state to the state – corresponding to two-photon occupation of the first (driven) cavity – are highlighted. The UPB is essentially based on suppression of such double occupation by a careful tuning of the model parameters, leading to destructive quantum interference between the two alternative pathways. The optimal UPB conditions Bamba2011 () are given by , and , and will be assumed to hold in what follows.
We consider the UPB mechanism in a SOI nanophotonic platform, where the cavity-field confinement in a diffraction-limited mode volume, , enhances the effective photon-photon interaction, . A realistic order of magnitude estimate in a crystalline silicon photonic crystal nanocavity leads to eV (see also Supplementary Information) Ferretti2013 (). Assuming a quality factor – now routinely achieved at telecom wavelengths (i.e., eV) Lai2014 (); Notomi2010 (); Sekoguchi2014 () – we set eV, and hence . To fulfill the optimal UPB conditions, the remaining parameters take values and , respectively.
The steady state results under cw driving are summarized in Fig. 1c-f. The time-dependent normalized second-order correlation function, (see Methods section) is considered as the reference figure of merit for single-photon blockade Birnbaum2005 (); Faraon2008 (); Reinhard2012 () and plotted in Fig. 1c. A strong antibunching is present over a time-delay window ps. At longer delays, strong oscillations are present on the timescale , arising from the interferential nature of the UPB mechanism Bamba2011 (). The average photon occupations in the two cavities, , and the corresponding zero-delay correlation, , are displayed as a function of the driving field amplitude, , in Fig. 1d: UPB occurs at low average occupation of the driven cavity, while the occupation of the non-detected cavity is much larger (see inset). This figure of merit is relevant to determine the maximal single-photon emission rate that can be achieved in such a device under cw pumping, given by . As an example, for (corresponding to and ), MHz can be expected, with an input power as low as nW. In fact, the optimal UPB relation between and leads to a condition (without numerical pre-factors, for convenience) ; this means that the required input-power in UPB scales down roughly as , i.e. the larger the cavity Q, the smaller can be to have antibunching by keeping the average number of photons in the first cavity less than 0.1 (according to Fig. 1d). The same figure of merit simultaneously allows to increase the antibunching time window, scaling as (see Fig. 1c).
Single-photon sources on demand require the emission of single-photon pulses at deterministic times. However, in the UPB mechanism the emitted light is sub-Poissonian only within a time delay shorter than , as shown in Fig. 1c. For short input pulses, the outgoing pulses will last at least as long as the cavity lifetime. Therefore, the condition would apparently prevent the device from operating in a pulsed regime Bamba2011 ().
Here we show for the first time that UPB under pulsed excitation is possible by exploiting temporal filtering of the output signal. In Fig. 2, the results of a numerical experiment are reported for the UPB device considered in the previous section, where a train of gaussian pulses drives the first cavity (Fig. 2a-c). A sequence of outgoing pulses from cavity 1 is modeled by solving the quantum master equation (see Supplementary Information for details), and shown in Fig. 2c. Focusing on a single outgoing pulse, the equal-time second-order correlation is plotted in Fig. 2d (blue curve), where a well-defined time window clearly exists – within the pulse emitted from a UPB device – during which light is antibunched over a time delay shorter than .
As a consequence, pulsed operation can be achieved by gating the outgoing pulses in time, in order to retain only a timeframe of duration . In practice, this could be achieved with an integrated all-optical switch triggered by the input pulse, as it was already shown experimentally Ates2013 (). The second-order correlation function under pulsed excitation (see Supplementary Information) is shown in Figs. 2e-g. The histograms in Figs. 2e-f show the un-normalized correlation signal, , integrated over the whole pulse sequence in (Fig. 2e) and in the presence of filtering with a time window ps (Fig. 2f), respectively. They reveal a strong reduction of the two photon counts within a pulse after filtering, which is a key result of this paper. Figure 2g displays the dependence of the filtered second-order correlation versus the filtering time window, . The Montecarlo data (blue disks), directly obtained from the photon count statistics (see Supplementary Information), are reproduced by a master equation treatment (cyan curve), which confirms the reliability of this result. Photon antibunching (gray area) is achieved below ps, while the single photon regime – requiring the condition – is obtained for ps. When assuming pulses per second and a peak value , after the temporal filtering the Montecarlo data indicate a single-photon yield at a rate of about 0.45 MHz. Under these conditions, the driven cavity reaches a peak value of the average photon occupation , close to the largest occupancy for which UPB is expected according to Fig. 1c [i.e., ]. Remarkably, this peak value of implies an intracavity energy of less than fJ per pulse. This corresponds to an input energy that can be quantified as fJ per pulse, according to typical excitation schemes of photonic crystal integrated circuits Dharanipathy2014 (). We notice that this is extremely low when compared to the state-of-art parametric sources demonstrated so far in integrated silicon-based platforms and based on four-wave mixing and heralding (typical input powers in the 100 mW range), for a comparable output rate in the few 100 kHz range Davanco2012 (); Spring2013b (); Thompson2013 ().
A feasible realization is hereby proposed in an integrated SOI photonic crystal platform. These structures benefit from a remarkably advanced and well established fabrication technology, with nanocavities having recently achieved -values well above the UPB requirements Lai2014 (); Dharanipathy2014 (); Notomi2010 (); Sekoguchi2014 (). As a schematic example, we show in Fig. 3a a double-cavity device in a photonic crystal circuit. This configuration allows to selectively drive one cavity from the input waveguide channel, and simultaneously collect part of the light emitted from the same cavity into the output waveguide (the remaining part being emitted through out-of-plane losses). As an elementary building block, we consider a L3 photonic crystal cavity in a thin silicon membrane, designed for operation at the preferred telecom wavelength, m ( eV). The cavity consists of three missing air holes in a triangular air-hole lattice. This cavity was recently optimized to show a measured quality factor regularly exceeding one million Lai2014 (); Minkov2014 (). We use here a L3 cavity design with theoretical unloaded (i.e., valid for the isolated cavity) (see Supplementary Information for details on the structure parameters, such as hole radius and lattice constant). When coupling to the access waveguides, the loaded Q-factor can be engineered in the range , as we have verified by 3D finite-difference time-domain simulations (3D-FDTD, not shown). From the calculated mode profile, the effective nonlinearity for this device is estimated (see Supplementary Information) in the range eV, close to what was assumed in the model calculations above.
The photonic crystal molecule can be obtained by vertically aligning two L3 cavities, separated by 5 rows of holes (i.e., center-to-center) Chalcraft2011 (). The hole radius in the central row, , can be varied to fine tune the normal modes splitting at the desired value Haddadi2014 (), i.e. according to Eq. 1 in Methods. In Fig. 3b we show such a simulated fine tuning by 3D-FDTD calculations. For nm, the normal mode splitting between the two resonances, identified as bonding (B) and antibonding (AB) according the the spatial profile of the component, is calculated as eV, i.e. remarkably close to the condition assumed in the previous calculations, when we consider the loaded value eV. We notice that similar values and dynamic control of the normal mode splitting have been already shown experimentally in SOI photonic crystal platforms operating in a very similar wavelength range Sato2012 (). The spectrum for such an optimal structure is shown in Fig. 3c. The two resonances have unbalanced Q-factors of (AB) and (B), respectively, which can also be exploited to enhance the degree of antibunching in UPB Ferretti2013 ().
Before concluding, we discuss how to circumvent the most relevant and potentially detrimental effects for the realization of UPB in a SOI platform. First of all, two-photon absorption (TPA), related to the imaginary part of the silicon , is also enhanced by confinement in the L3 cavities. However, a quantitative estimate of this contribution has been given in Ref. Ferretti2012, , by which we can infer a TPA loss rate that is on the order of for the present case, also considering the low input powers necessary to achieve UPB. Second, thermal effects can give rise to pure dephasing of the cavity resonances, which depends on optomechanical coupling with the background phonons. For the L3-type silicon photonic crystal cavities considered here, this contribution has been quantitatively estimated and shown to be negligible even at room temperature (i.e., a pure dephasing rate ) Flayac2014 (). Finally, unavoidable fabrication imperfections should be corrected by device post-fabrication processing. In particular, fine and selective cavity tuning has been already shown for photonic crystal cavities with different techniques, even in the presence of very large Q-factors Sato2012 (); Caselli2013 (); Waks2013apl ().
We have theoretically shown that an integrated nanophotonic platform based on CMOS-compatible SOI technology can be engineered to achieve single photon emission by an unconventional photon blockade mechanism. Besides opening the way to the first experimental demonstration of UPB, our results show that such unconventional mechanism allows for pulsed excitation, which represents a key ingredient for a useful source where each pulse potentially triggers emission of a single photon.
Such an alternative single-photon source could be characterized by a very low input power operation, i.e. comparable to standard single-photon devices based on cavity QED but much lower than typical integrated single-photon sources based on enhanced four-wave mixing and heralding. Moreover, this is achieved by an unprecedented small footprint area, significantly smaller than recently realized heralded sources in integrated SOI chips. In fact, notice that the footprint of this prospected device is essentially given by the spatial extension of the photonic crystal molecule and the necessary lattice around it. For the structure simulated in Fig. 3, we estimate a minimal footprint area on the order of a few m (see, e.g., the inset in Fig. 3c). In practice, this is significantly smaller than current heralded sources fabricated with the same SOI technology and based on coupled resonator optical waveguides Davanco2012 () or spatially multiplexed photonic crystal waveguides Collins2013 (). We also stress the generality of the proposed scheme, which could be extended to other types of nonlinearities Gerace2014 (), and could eventually lead to the realization of novel quantum devices Gerace2009 (); Dudu2014 () for applications in integrated quantum metrology and logic.
In summary, by combining an extremely low input power, a small footprint area, and no quantum emitter required for single-photon generation, such a device might have significant impact on the development of integrated silicon quantum photonics, by introducing a new concept in the generation of pure quantum states of light at arbitrary wavelengths (e.g., in the telecom band), that is fully compatible with current semiconductor technology, working at room temperature, and a viable alternative to single-photon nonlinear devices based on cavity-QED with artificial atoms or single atomic-like emitters that are presently lacking in SOI integrated platforms.
Model Hamiltonian. The second quantized hamiltonian of the driven nonlinear photonic molecule is expressed (to leading linear and nonlinear orders) as Liew2010 (); Bamba2011 (); Ferretti2013 ()
The first terms in Eq. 1 describe two harmonic oscillators, is the tunnel coupling rate between the two resonators, is the coherent pumping rate on the first cavity at the laser frequency , and the photon-photon interaction energy in each resonator is related to the material Ferretti2012 (); Ferretti2013 (). A description of this quantity and an estimation for the photonic crystal cavities considered here are given in the Supplementary Information. Starting from this Hamiltonian, the various time-dependent photon correlation functions for light collected after cavity 1, generally defined as
were numerically simulated by using both the Montecarlo wave function method and by directly solving the master equation for the density matrix (see details in Supplementary Information). In both cases, the numerical solutions were computed on a truncated Hilbert space of dimensions , where and are the maximum photon occupations allowed in cavities 1 and 2, respectively. While the master equation results were obtained from a modern workstation embedding 16 Gb of RAM, the Montecarlo data were produced by 10 nodes of 16 cores and 32 Gb RAM memory each, run on a high-end cluster for a few weeks of continuous computational time.
Several useful discussions with A. Badolato, I. Carusotto, S. Ferretti, M. Galli, A. Imamoǧlu, T. F. Krauss, T. C. H. Liew, L. O’Faolain, K. Srinivasan, H. E. Türeci, and J. P. Vasco, are gratefully acknowledged. The authors acknowledge the Swiss National Science Foundation for support through the International Short Visits program, project number IZK0Z2-150900. D.G. acknowledges partial financial support from the Italian Ministry of University and Research through Fondo Investimenti per Ricerca di Base (FIRB) “Futuro in Ricerca” project RBFR12RPD1.
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Supplementary Information to
“An all-silicon single-photon source by unconventional photon blockade”
We detail here the Montecarlo and master equation treatments used to produce the results of figures 1 and 2 in the main text. We also give details on the photonic crystal cavities design, and the corresponding estimation of the single-photon nonlinearity reported in the manuscript.
Appendix A Montecarlo wave function method
The statistics of the photons emitted by the system under pulsed excitation were first addressed by performing quantum Montecarlo simulations Dum1992 (). This method not only allows to work with larger truncated Hilbert spaces but also provides direct access to individual photon counts, thus embodying the closest theoretical simulation of an actual Hanbury Brown-Twiss experiment. In brief, the algorithm is based on the stochastic evolution of the system wave function through the Schrödinger equation
written for the non-Hermitian effective Hamiltonian
The non Hermitian part of 2 results in a decay of the norm . During the evolution of Eq. 1, random numbers are drawn and the condition decides for the action of a jump operator, , corresponding to the measurement of a photon. The proper quantum jump operator is chosen such that is the smallest integer satisfying , where are the probabilities for the mode to emit a photon at a given time. Each evolution of Eq. 1 produces a stochastic quantum trajectory associated with the state , and the procedure can be repeated times to form an ensemble average of realizations in view of approximating the system density matrix as , where
and its potential mixed nature. Any observable or correlation are obtained from . The full access to photon counts and emission times history allows to mimic the experimental detection scheme. The two-times second-order correlation function, , can be reconstructed from the statistics of photons delays analogously to a Hanbury Brown and Twiss (HBT) setup. Further details on the numerical procedure employed to obtain the results of Fig. 2 in the main text are given in the following.
Appendix B Two-time correlations under pulsed excitation
In our Montecarlo simulations we have worked on the basis of trajectories containing single pulses, which makes the data analysis more flexible. We have tracked the quantum jumps performed by the driven cavity from which the photon antibunching is expected. We point out that in reality one should expect a weak mixing between both cavity fields to occur in the guiding channels. It can be accounted for within an input-output treatment. In such a case the laser detuning should be properly adapted according to the prescriptions of Ref. Flayac2013, . To analyze delays within a given pulse we need to track the trajectories where at least two quantum jumps occurred within and these events are obviously rare given the relatively small occupation of the cavity 1 as one can see from Fig. 2 of the main text. We have therefore performed a large campaign of massively parallelized simulations on an high end cluster based on pulses from which we have recorded the whole quantum jump history. We considered pulses of duration 4 ns separated by 20 ns to avoid any overlap bringing some unwanted pulse to pulse correlations. Our simulation therefore covers not less than 1 seconds of recorded data.
To build the Monte-Carlo curve of Fig. 2g (blue disks), we have worked on quantum jumps that occurred in a time window of width ns centered on the minimum (see yellow surface and blue curve of Fig. 2f) mimicking the temporal filtering. Inside this global window we have considered sub-windows of variable duration ranging from 6.5 ps to . Each of these sub-windows was gradually displaced by within , starting from the condition () and until () is fulfilled. For a given value of , the un-normalized second order correlation is obtained from the sum of photon pair counts recorded by slicing the time window, which increases the statistics by . Therefore it allows to work with a number of counts that would correspond to trajectories (pulses) reducing by the required computational time. Finally, the is obtained by normalizing to the number double counts expected from a Poissonian statistics. The errors (magenta curve) are computed from the square root of the number of counts averaged over the sliding windows. Obviously the error is inhomogeneous versus , given that is variable, and it is small both in the regions of narrow and wide where respectively is large and number of counts is important. The previously described procedure is summarized in Fig. S1 (see captions).
To build the histograms of Fig. 2d-e displaying the pulse-to-pulse statistics, we have performed a Montecarlo rearrangement of our single pulse trajectories to randomize their time ordering, as it would be obtained from many pulse trajectories or in an actual experimental situation.
Appendix C Quantum master equation
The master equation for the density matrix reads
where losses are accounted for through Liouvillian operators in the usual Lindblad form for the two resonators modes, . Further sources of loss, such as nonlinear absorption (e.g. related to the imaginary part of ) or pure dephasing, could also be added to Eq. 4 (see, e.g. Ferretti2012, ; Ferretti2013, ), but we neglect them here for simplicity. Moreover, the model can be generalized to include input and output quantum channels Flayac2013 ().
Single-time evolution and steady state numerical results of Eq. 4 can be straightforwardly performed, as in Refs. Liew2010, ; Bamba2011, ; Ferretti2013, . Here, we were additionally able to confirm the Montecarlo results (cyan curve in Fig. 2g of the main text). The un-normalized and normalized two-times second-order correlation functions of cavity 1 were computed as
where is the propagator of the operator from to associated with Eq. 4. The photon statistics produced within a time window is obtained from
where . This exact calculation perfectly reproduces the Montecarlo wave function results within the error envelope, as it is reported in Fig. 2g (cyan curve).
Appendix D Photonic crystal cavities design
Photonic crystal cavities allow to achieve record figures of merit today, such as ultra-small mode volumes and ultra-high quality factors Notomi2010 (). One of the most used photonic crystal cavity designs is realized by removing three air holes in a triangular lattice Akahane2003 (), which is usually defined a L3 point defect. Recently, a combination of fast simulation tools Andreani2006 () and genetic optimization Minkov2014 () have allowed to show that Q factors largely exceeding can be designed for such cavities, which was shown experimentally Lai2014 ().
For the photonic crystal cavities design used in this work, we started from a standard SOI photonic crystal membrane, with the silicon layer thickness of 220 nm. We set the lattice constant to nm and the holes radius to nm () to tune the cavity mode resonant wavelength in the relevant telecom band, i.e. m ( eV). The three holes along the cavity axis have been shifted by nm () nm (), and nm (), to reach a theoretical (unloaded) . Since we aim at coupling these cavities with access and output waveguides, we thus allow the loaded Q-factor to be in the range.
A plot of the normalized electric field intensity, i.e. .the function with , is shown in Fig. S2 for our optimized L3 cavity design, which was the building block for the the photonic crystal molecules in Fig. 3 of the main text.
Appendix E Estimating the effective photon-photon interaction
In this work, we focus on photonic nanostructures in silicon, which is a strongly nonlinear material already at the level of classical electromagnetic response. In particular, bulk silicon is characterized by a relatively large susceptibility, while nominally (neglecting surface contributions) owing to the centrosymmetric nature of the elementary crystalline cell Boyd2008 (). Strongly enhanced nonlinear effects have been already reported in L3 photonic crystal cavities Galli2010 ().
The photon-photon interaction energy in each resonator is given in terms of the material by the simplified expression Ferretti2012 ()
where is the three-dimensional cavity field profile, normalized as , and represents the multiple contributions of the same order of magnitude given by the different elements of the tensor Boyd2008 ().
From the calculated mode profile shown in Fig. S2, the effective nonlinearity of such a silicon nanocavity can be estimated through Eq. 8, by using mV, which is an appropriate order of magnitude for the elements of the bulk silicon third-order susceptibility tensor Boyd2008 (), and D=24 Sipe1987 (). For the cavity mode profile of our optimized photonics crystal structure, see Fig. S2, a quantitative estimate of this integral results in eV, close to what was assumed in the model calculations of the main text and confirming the order of magnitude estimates already given in the literature Ferretti2013 ().
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