Nature Physics  Letter
Weakvalue amplification of the nonlinear effect of a single photon
 Matin Hallaji^{1}^{, }
 Amir Feizpour^{1}^{, }
 Greg Dmochowski^{1}^{, }
 Josiah Sinclair^{1}^{, }
 Aephraim M. Steinberg^{1, 2}^{, }
 Journal name:
 Nature Physics
 Volume:
 13,
 Pages:
 540–544
 Year published:
 DOI:
 doi:10.1038/nphys4040
In quantum mechanics, the concept of weak measurements allows for the description of a quantum system both in terms of the initial preparation and the final state (postselection)^{1}. This paradigm has been extensively studied theoretically and experimentally, but almost all of weakmeasurement experiments carried out to date can be understood in terms of the classical (electromagnetic wave) theory of optics. Here, we present a quantum version in which the measurement apparatus deterministically entangles two distinct optical beams. We show that a single photon, when properly postselected, can have an effect equal to that of eight photons: that is, in a system where a single photon has been calibrated to write a nonlinear phase shift of ϕ_{o} on a probe beam, we measure phase shifts as large as 8ϕ_{o} for appropriately postselected single photons. This opens up a new regime for the study of entanglement of optical beams, as well as further investigations of the power of weakvalue amplification for the measurement of small quantities.
Subject terms:
At a glance
Figures
Main
Measurement of a property of a system generally proceeds by coupling the system to a probe in such a way that the change of state of the probe depends on the value of this property. For example, a galvanometer is constructed so that its needle deflects by an amount proportional to the potential difference across the system being studied. A subsequent observation of the final state of the probe provides information (often incomplete) about the value of the observable. In quantum mechanics, this information is gained at the price of disturbing the system through the interaction. There is a strict tradeoff between the minimum disturbance and the amount of information which can be gained^{2, 3, 4}. In weak measurement, the disturbance to the system is reduced at the cost of a similar reduction in the amount of information provided by the measurement. This minimal disturbance makes it reasonable to consider conditioning the readout of the probe on finding the system in a particular final state after the interaction (postselection). In this case, the pointer shift, averaged over many measurement repetitions, has been shown^{1} to have a magnitude which would correspond to what is termed the ‘weak value’ of the observable: , where is the observable, and i and f are the pre and postselected states of the system, respectively. Evidently, the weak value depends equally on both preselected (initial) and postselected (final) states. This feature of weak measurement makes it a powerful tool for exploring fundamental questions in quantum mechanics^{3, 5, 6, 7, 8, 9, 10, 11, 12, 13, 14, 15, 16}, specifically the properties of postselected subensembles ranging from particles transmitted through tunnel barriers to measurementbased quantumcomputing systems^{17, 18, 19}.
Strangely, the weak value is not constrained to be within the eigenvalue spectrum of the observable , and is not even in general a real number. In particular, as the overlap between the initial and final states becomes very small, fi 0, the weak value can become (almost) arbitrarily large (as long as the postselection success is dominated by the overlap of pre and postselected states and not the measurement backaction; see the Supplementary Information.) Indeed, the founding paper of the field^{1} appeared under the unwieldy but provocative title ‘How the result of a measurement of a component of the spin of a spin1/2 particle can turn out to be 100’. This has led to the idea of using ‘weakvalue amplification’ (WVA) to improve the detection or measurement of small effects^{20, 21, 22, 23, 24, 25, 26}. Interest in this application of weak measurement has grown in the past few years alongside an ongoing debate on the usefulness of WVA^{27, 28, 29, 30, 31}. Even the quantum mechanical nature of WVA has been challenged^{32}, and attempts have been made to describe the effect classically based on measurement disturbance. In 2011, we proposed that WVA of the small optical nonlinearity at the singlephoton level^{33} was possible and could, under some conditions, improve the signaltonoise ratio. Here, we present an experiment implementing this idea, asking a question directly analogous to that of the original Aharonov, Albert and Vaidman paper: In a twoarm interferometer containing one photon in total, can the result of a measurement of the photon number in one arm turn out to be greater than 1? We find the answer is yes.
Anomalous weak values observed to date^{20, 21} have typically utilized two different degrees of freedom (such as polarization and propagation direction) of a photon as the ‘system’ and the ‘probe’, obviating the need for any interphoton interaction; the effects can thus be explained perfectly in terms of linear optics, without resorting to quantum theory. There have been two exceptions. In one, a probabilistic quantum logic gate was implemented, so that although there was no deterministic entanglement of system and probe, an additional postselection step projected the system onto an entangled state some fraction of the time^{14, 34}. In the other, deterministic WVA was implemented in a transmon qubit system^{35}. Here, we present the first observation of WVA via deterministic entanglement of two distinct optical systems, amplifying the number of photons in a signal beam by measuring the nonlinear phase shift it writes on a separate probe beam. From the perspective of the development of quantum nonlinear optics, this is exciting evidence for, and an application of, the deterministic entanglement between two independent light beams at the quantum level, which can now be generated thanks to modern techniques for enhancing nonlinearities. By contrast with the transmon work, in which entanglement occurs between two stationary qubits on a single chip, our observations rely on entanglement between two distinct light beams propagating in opposite directions, which are eventually measured on two different detectors which are about a metre apart, and could in principle be arbitrarily distant from each other.
In 2011, we proposed that WVA could be used to amplify the (weak) nonlinear effect of photons in a signal pulse on a probe beam. The scheme begins by splitting the signal beam into two paths (Fig. 1), which are later interferometrically recombined such that there is strong constructive interference at one port, and very few photons exiting the other, ‘nearly dark’, port. By postselecting on cases where a photon exits this nearly dark port, one can ‘amplify’ the weak value of the photon number in one arm of the interferometer. The physical content of this statement is that if an optical probe beam interacts, through a Kerrtype nonlinear medium, with the light in that arm of the interferometer, it will experience a phase shift proportional to the weak value of the photon number, which may be much larger than the nonlinear phase shift expected for a single signal photon—even if there was only ever a single signal photon present in the entire interferometer.
In our experiment, the nonlinear interaction between the signal and probe beams is mediated by a sample of lasercooled ^{85}Rb atoms in a magnetooptical trap (MOT). A coupling beam is used to set up electromagnetically induced transparency (EIT) for the probe beam. The frequencies of the probe and coupling beams are set so that each of them is individually on resonance with its corresponding atomic level (Fig. 2b). The EIT resonantly enhances the nonlinear interaction between the signal and the probe beams, while simultaneously minimizing the probe absorption. As a signal pulse passes through the medium, it alters the optical properties (the index of refraction) of the medium as seen by the probe beam. As a result of this change in the index of refraction, the probe picks up a phase shift relative to what the phase would have been in the absence of the signal pulse. This cross phase shift (XPS) depends linearly on the number of photons (intensity) of the signal pulse^{36}. This interaction thus constitutes a measurement of signal photon number, with the phase of the probe beam acting as a ‘pointer’. The typical phase shift per photon is on the order of 10^{−5} rad (ref. 36), much smaller than the quantum uncertainty in our probe phase, meaning that a single measurement cannot provide enough information to determine the photon number to better accuracy than its initial uncertainty, which is the sense in which this measurement is ‘weak’.
The geometry and polarizations of the coupling and probe beams (Fig. 2) are chosen such that the strength of this nonlinear interaction also depends on the polarization of the signal beam, with the interaction being strongest for righthanded circular (σ^{+}) polarization and weakest for lefthanded circular (σ^{−}) polarization of the signal; see Supplementary Information. As mentioned before, an interferometer is necessary to implement WVA of signal photon number. We chose this configuration so as to use the polarization dependence of XPS to build an interferometer for the signal beam, in which the two ‘paths’ of the interferometer are in fact two polarizations, to one of which the probe beam is much strongly coupled than to the other (Fig. 2). The incident signal photons are linearly polarized—that is, in an equal superposition of σ^{+} and σ^{−}. After they interact with the probe beam, we use a waveplate and a polarizer to transmit photons with a nearly orthogonal polarization (corresponding to the nearly dark interferometer port, Fig. 1), which subsequently impinge on a singlephoton counting module (SPCM). When this detector fires, constituting a successful postselection, a large weak value of photon number (and hence large nonlinear phase shift) is expected; for each signal pulse, we record whether or not the detector fires, to measure the average nonlinear phase shift written on the probe separately for the cases of successful postselection (which we term ‘click’) and the cases of failed postselection (‘noclick’).
Although our original proposal concerned a signal pulse that contained a singlephoton Fock state^{33}, a similar effect can be observed even if one uses a coherent state, with an average photon number larger than one. In that proposal we showed that the weak value of photon number in one arm of the interferometer, when the photon is postselected to be in the nearly dark port, is given by n_{wk} = 1/2 + 1/2δ. The parameter δ is defined as the overlap between the initial and final state of the photon, ranging from 0 (completely dark port) to 1 (bright port). However, here δ is assumed to be very small, which corresponds to a nearly dark port. In another work^{36}, we showed that, in the limit of low detection efficiency, the (mean) inferred photon number in a coherent state containing photons, when conditioned on a successful photon detection, increases by one photon: the inferred photon number after a successful postselection, n_{click}, turns out to be one more than the inferred photon number in the absence of a click, n_{noclick}. Now, if one combines these ideas, sending a coherent state in the interferometer instead of a singlephoton Fock state and conditioning the photon number measurement of one arm on detection of a photon in the nearly dark port, the added photon due to the photon detection will undergo weakvalue amplification. Using B and D to denote bright and nearly dark ports, one can approximate the initial signal coherent state i ≈α_{B} αδ_{D} as α_{B} (0 + αδ1)_{D}, and the final state postselected when the detector fires as α_{B} 1_{D} (occurring with probability α^{2}δ^{2}, multiplied by the experimental collection and detector efficiency.) One can then calculate the weak value of the number of photons in each arm of the interferometer, n_{±}_{wk}, with ‘plus’ and ‘minus’ signs denoting the σ^{+} and σ^{−} polarizations, by
The number operators can be written a_{±}^{†}a_{±}, where the field operators . The numerator can thus be written
As the denominator simply evaluates to δ, we find
(See the Supplementary Information for a more detailed derivation of equation (3).) It is instructive to note that the total number of photons inside the interferometer is , where is the average number of photons sent into the interferometer, and is the revised estimate of the mean photon number based on detection of one ‘additional’ photon in the nearly dark port. What equation (3) demonstrates is that this added photon (‘the’ photon which causes the SPCM in the nearly dark port to fire, so to speak) undergoes WVA, giving rise to the term 1/2δ. This occurs even in the presence of a ‘background’ of nonpostselected photons. The firing of the detector alerts us to the fact that a single photon reached the postselection port, and the effect of that photon on the probe is consequently amplified; on the other hand, it provides no additional information about the behaviour of the other n photons, each of which therefore exhibits a 50% probability of being in the correct arm to affect the probe beam. This 50% is determined entirely by the preparation, as the undetected photons undergo no postselection, and their effect is not amplified. In this context, when the probe beam interacts with the one arm of the interferometer, the nonlinear phase shift written on it will be proportional to the weak value of photon number in that arm. Due to the spatial overlap between the probe beam and the two arms, which are the two circular polarizations of the signal beam, the total XPS written on the probe is ϕ = n_{+}_{wk}ϕ_{+} + n_{−}_{wk}ϕ_{−}, where ϕ_{±} are the perphoton phase shifts for the corresponding signal polarizations. On detection of a photon in the nearly dark port (a click event), these are to be replaced by the weak values from equation (3), leading to . The amplification shows up in the second term, which is proportional to the difference between the XPS for the two polarizations. In cases when the detector fails to detect a photon (noclick events), there is no ‘added photon’ and the weak value of photon number in each arm is simply , corresponding to an XPS of .
Figure 3 shows the measured XPS for the click and noclick events versus a range of values of postselection parameter δ; for each δ, the mean input photon number and the overall detection efficiency η are adjusted so as to keep the probability of photon detection ( ) low, which is the necessary condition for a photon detection to add one photon to the inferred photon number^{36} (for more technical details see the Supplementary Information.) The measured XPS for the click events is manifestly always larger than the measured XPS for the noclick cases. It is worth noting that had we not utilized postselection to separate the click from noclick events, the expected XPS of the probe would have been , which is the same as ϕ_{noclick} when the overall detection efficiency is low. Therefore, we can define ϕ_{0} = (ϕ_{+} + ϕ_{−})/2 as the expected perphoton phase shift for this experiment. The inset of Fig. 3 plots ϕ_{noclick} versus the input photon number. From a linear fit to this data, the perphoton phase shift ϕ_{0} is measured to be 5.59 ± 0.02 μrad.
To directly observe the WVA of the added photon due to photon detection, we plot ϕ_{click} − ϕ_{noclick} versus the postselection parameter δ in Fig. 4. It is easy to see that this quantity, which we term ‘the differential phase shift’, is independent of , and contains only the XPS of the added photon and its amplified effect: ϕ_{click} − ϕ_{noclick} = (ϕ_{+} + ϕ_{−})/2 + (1/δ)(ϕ_{+} − ϕ_{−})/2. The plot clearly shows that, as δ becomes smaller, the effect of the postselected single photon becomes larger. For δ = 0.1, the smallest postselection parameter used in our experiment, we measure a differential phase shift of 47.0 ± 13.5 μrad, which is 8.4 ± 2.4 times larger than the perphoton phase shift ϕ_{0}. Hence, a single postselected photon can act like eight photons. In an ideal case, where only the photon number in one arm of the interferometer is measured, δ = 0.1 corresponds to an amplification factor of ten. For the points with δ = 0.14 and δ = 1, we used nearly the same mean photon number (45 and 40, respectively), so that the results would be directly comparable even without knowledge of the independence of the differential phase shift on . For the δ = 1 case, we observed 6.7 ± 7.5 μrad, consistent with the unamplified value of 5.59 ± 0.02 μrad expected in the absence of WVA, while for the δ = 0.14 case we found 34 ± 10 μrad, three standard deviations above ϕ_{0}. From a fit to the data in Fig. 4 we estimate ϕ_{+} − ϕ_{−} to be 8.7 ± 0.6 μrad.
Given the extensive discussion in recent years over the possible merits of WVA for making sensitive measurements of small parameters, it is interesting to contrast the present experiment with an earlier one, in which we measured the nonlinear phase shift due to postselected single photons, but without any weakvalue amplification^{36}. In our previous experiment, a total of approximately 1 billion trials (300 million events with postselected photons, and 700 million without) were used to measure the XPS due to σ^{+}polarized photons. By looking at the difference between the XPS measured for ‘click’ and ‘noclick’ events, we measured peak XPS ϕ_{+} of 18 ± 4 μrad. In this experiment, where we use the WVA technique, we used a total of around 830 million trials (200 million successful postselections) to extract an average XPS ϕ_{+} of 10.0 ± 0.6 μrad (for more information regarding the reported average XPS see the section entitled ‘Probe phase measurement’ in the Supplementary Information). Note that this number agrees well with our classical calibration of the peak XPS of 13.0 ± 1.5 μrad^{36}. It is evident that the WVA technique yielded a better signaltonoise ratio (SNR). This may seem surprising at first, given that under statisticalnoise conditions, WVA is known to have the same SNR as a bruteforce measurement^{33}; this is because the amplification of the signal only comes at the price of a postselection which reduces the size of the data set just enough to cancel out any advantage one might have hoped for. In our case, however, while the differential phase shift grows as 1/δ, the size of the postselected data set is determined by . Hence, we were able to maintain a substantial set of postselections even for small δ simply by adjusting accordingly. This allowed us to amplify the perevent signal while keeping the number of events high, thereby achieving a precise measurement of the differential phase shift. Furthermore, in the noclick cases, the large photon number provided an excellent determination of ϕ_{0}. Therefore, we were able to estimate the value of ϕ_{+} more precisely with fewer trials. It is essential to note that the WVA technique in this experiment is advantageous only if one considers the number of trials (and not the number of photons) as the measurement resource.
Future work will address the ongoing discussions about the advantages of WVA over traditional strong measurement. To tackle this question, future iterations of the experiment can be carried out with artificial noise added, conforming to a variety of noise models. It is expected that in cases where the noise has long time correlations, WVA will prove superior to standard measurement for the estimation of small parameters such as the intrinsic perphoton phase shift or χ^{(3)} of a sample.
Methods
Atom preparation.
A cloud of ^{85}Rb atoms is prepared in a magnetooptical trap (MOT). Three pairs of beams are used for cooling while a magnetic gradient of approximately 20 G cm^{−1} (along the quadrupole axis) provides confinement in space. Each beam contains a trapping beam, tuned 20 MHz to the red of the F = 3 F′ = 4 transition, and a repumper, which is tuned close to the F = 2 F′ = 3 resonance. Each measurement cycle lasts for 52 ms. For the first 50 ms, the MOT beams and magnetic field gradient cool and prepare the cloud. They are then turned off and the atoms are probed for 1.5 ms with a 500 μs gap between cooling and probing to ensure the absence of residual magnetic field gradients.
Probe phase measurement.
To measure the phase and amplitude of the probe beam, we use frequencydomain interferometry. The probe beam is comprised of two frequency components that copropagate through the interaction region. One frequency component is tuned to resonance with F = 2 F′ = 3. A second frequency component is prepared by frequencymodulating an acoustooptic modulator (AOM) at 100 MHz, and is used as a probe reference. The beating of these two components is detected on a fast avalanche photodiode. Any change in the phase and/or amplitude of the probe beam results in a change in phase and/or amplitude of this 100 MHz beating signal. We use an IQdemodulator to then read off the phase (arctan(I/Q)) and amplitude ( ) of the beat signal. The resulting phase and amplitude are digitized with a sampling period of 200/3 ns (sampling frequency of 15 MHz). Each measurement cycle contains 22,501 samples (corresponding to 1.5 ms of phase measurement), which we call a trace. The first 4,500 samples (300 μs) in each trace are ignored to avoid contamination from the residual probe phase dynamics. The last 180 samples are used to measure the final OD of the atomic cloud (by turning the coupling beam off, hence eliminating the EIT, and measuring the probe absorption). The remaining 1.188 ms is divided into 495 shots, 2.4 μs (36 samples) each. Each shot contains a nonlinear phase shift due to the interaction between the probe and the signal pulse. The nonlinear phase shift has a fullwidth at halfmaximum width of around 500 ns (ref. 37). We average the value of this phase shift for seven samples (466.6 ns) in each shot. To eliminate slow drifts in our phase measurement, the phase of the probe is averaged for three samples (200 ns) with a 266 ns gap before and after the seven samples. This value is then subtracted from the average of the probe phase in the interval when nonlinear phase shift is expected. The resulting number represents the average phase shift due to the signal pulses, and is reported as the measured XPS. It is worth noting that the reported values for XPS in this report underestimate the peak phase shift because of the averaging and background subtraction. The probe beam contains about 2,000 photons, which corresponds to a 11 mrad quantum limit on the phase uncertainty (shotnoise). We determine our phase uncertainty experimentally by calculating the standard deviation and the standard deviation of the mean from our data sets. The standard deviation is about 100 μrad, which is about ten times larger than the quantum limit on the phase uncertainty. To measure the phase shift down to a few μrad precision, we repeat the measurement about half a billion times with around 200 shots in each 1.5 ms measurement window. The final reported uncertainty is the standard deviation of the mean of this full data set.
Probe and coupling fields.
Electromagnetically induced transparency (EIT) is a coherent effect in which destructive interference prevents the two laser beams from being absorbed by the atoms. To generate EIT, the probe and coupling lasers should be phaselocked. To generate the probe beam, some power is first extracted from a master laser beam that is locked approximately 30 MHz red of the F = 2 F′ = 3 transition. By using an AOM that is driven at + 130 MHz (doublepassing at + 65 MHz), the offresonance component of the probe beam is generated. This offresonance beam is then sent through another AOM at −100 MHz to generate the onresonance probe component. The two beams are then combined on a beamsplitter and sent towards the interaction region. We use an electrooptic modulator (EOM), which is driven at around 3 GHz, to frequency modulate the remaining portion of the master laser; this writes frequency sidebands on the laser. The frequency modulated beam is then used to seed an injectionlocked diode laser and we lock this diode laser to the first lower sideband. As a result, the second diode laser, the coupling laser, is phaselocked to the master laser. The frequency of the coupling beam is set to be on resonance with the F = 3 F′ = 3 transition. We use another AOM (singlepass driven at +103 MHz) to switch the coupling beam on and off. The intensities of the probe and coupling beams are chosen so that the resulting EIT width is 2 MHz. The polarizations of the probe and coupling beams are set to be σ^{+} and π respectively.
Signal pulses.
A portion of the injectionlocked diode laser, mentioned above, is sent though two AOMs. These AOMs are used to set the frequency of the pulses to be around + 18 MHz from the F = 3 F′ = 4 transition. One of the AOMs is also used to amplitudemodulate the signal beam to create 40 ns pulses. A neutral density (ND) filter is used to attenuate the signal pulses, preparing pulses with low average photon numbers. A polarizer followed by a halfwave plate and a quarterwave plate is used to set the polarization of the signal pulse before its interaction with the probe. For all WVA measurements reported here, the signal pulse is initially linearly polarized.
Signal postselection.
After its interaction with the probe beam, the signal beam is sent through a halfwave plate, a quarterwave plate and a Glan–Thompson polarizer. With this combination, the polarization of the signal beam is fully characterized with and without the atoms (by doing tomography). Once the initial polarization of the signal beam is well understood, and any polarization rotations due to the presence of atoms are corrected for, the half and quarterwave plates are set so that the signal polarization in the output of the Glan–Thompson polarizer is projected onto a polarization almost orthogonal to the initial polarization with real overlap with the initial polarization. The signal pulses are then collected in a multimode fibre and are detected on a SPCM. On detecting a photon, the SPCM sends a signal which triggers our tagging module to expose the probe detector to a 100 ns flash of light. This pulse shows itself as a spike in the probe amplitude and phase. This spike tags the corresponding shot as a successful postselection. A time delay between when the tag appears in a shot and when the XPS is expected to happen is introduced and carefully adjusted to avoid any incursion of the tags to the measured XPS in that shot. The tags, however, affect the XPS in the next shot and, therefore, the shot after each tag is discarded. We then use these tags, and the absence thereof, to group the shots into successful (click) and unsuccessful (noclick) postselection bins.
Background photons.
Any residual photon that hits the SPCM results in a photon detection which will falsely be counted as a successful postselection. To reduce the chances of getting a false positive, we timegate the SCPM in the 40 ns windows where we expect the signal pulses to arrive. With this gating, 6% of the measured shots are still falsely tagged as ‘click’. These background detections cause deterioration in the desired effect. Therefore, to be less sensitive to these detections, we attempt to operate in regimes where the total detection rate is 20–30%.
Data availability.
The data that support the plots within this paper and other findings of this study are available from the corresponding author upon request.
Change history
 Corrected online 06 March 2017
 In the version of this Letter orginally published, L. Vaidman's surname was spelled incorrectly in the second paragraph of the body text. This has now been corrected in all versions of the Letter.
References
 Aharonov, Y., Albert, D. Z. & Vaidman, L. How the result of a measurement of a component of the spin of a spin1/2 particle can turn out to be 100. Phys. Rev. Lett. 60, 1351–1354 (1988).
 Ozawa, M. Universally valid reformulation of the Heisenberg uncertainty principle on noise and disturbance in measurement. Phys. Rev. A 67, 042105 (2003).
 Erhart, J. et al. Experimental demonstration of a universally valid error–disturbance uncertainty relation in spin measurements. Nat. Phys. 8, 185–189 (2012).
 Rozema, L. A. et al. Violation of Heisenberg’s measurement–disturbance relationship by weak measurements. Phys. Rev. Lett. 109, 100404 (2012).
 Resch, K., Lundeen, J. & Steinberg, A. Experimental realization of the quantum box problem. Phys. Lett. A 324, 125–131 (2004).
 Kocsis, S. et al. Observing the average trajectories of single photons in a twoslit interferometer. Science 332, 1170–1173 (2011).
 Rozema, L. A. et al. Violation of Heisenberg’s measurement–disturbance relationship by weak measurements. Phys. Rev. Lett. 109, 100404 (2012).
 Lundeen, J. S., Sutherland, B., Patel, A., Stewart, C. & Bamber, C. Direct measurement of the quantum wavefunction. Nature 474, 188–191 (2011).
 Foster, G. T., Orozco, L. A., CastroBeltran, H. M. & Carmichael, H. J. Quantum state reduction and conditional time evolution of wave–particle correlations in cavity QED. Phys. Rev. Lett. 85, 3149–3152 (2000).
 Lundeen, J. S. & Steinberg, A. M. Experimental joint weak measurement on a photon pair as a probe of Hardy’s paradox. Phys. Rev. Lett. 102, 020404 (2009).
 Yokota, K., Yamamoto, T., Koashi, M. & Imoto, N. Direct observation of Hardy’s paradox by joint weak measurement with an entangled photon pair. New J. Phys. 11, 033011 (2009).
 Danan, A., Farfurnik, D., BarAd, S. & Vaidman, L. Asking photons where they have been. Phys. Rev. Lett. 111, 240402 (2013).
 Piacentini, F. et al. Experiment investigating the connection between weak values and contextuality. Phys. Rev. Lett. 116, 180401 (2016).
 Pryde, G. J., O’Brien, J. L., White, A. G., Ralph, T. C. & Wiseman, H. M. Measurement of quantum weak values of photon polarization. Phys. Rev. Lett. 94, 220405 (2005).
 Denkmayr, T. et al. Observation of a quantum Cheshire cat in a matter–wave interferometer experiment. Nat. Commun. 5, 4492 (2014).
 Murch, K. W., Vijay, R. & Siddiqi, I. Weak Measurement and Feedback in Superconducting Quantum Circuits 163–185 (Springer International Publishing, 2016).
 Steinberg, A. M. How much time does a tunneling particle spend in the barrier region? Phys. Rev. Lett. 74, 2405–2409 (1995).
 Knill, E., Laflamme, R. & Milburn, G. J. A scheme for efficient quantum computation with linear optics. Nature 409, 46–52 (2001).
 Raussendorf, R. & Briegel, H. J. A oneway quantum computer. Phys. Rev. Lett. 86, 5188–5191 (2001).
 Hosten, O. & Kwiat, P. Observation of the spin Hall effect of light via weak measurements. Science 319, 787–790 (2008).
 Dixon, P. B., Starling, D. J., Jordan, A. N. & Howell, J. C. Ultrasensitive beam deflection measurement via interferometric weak value amplification. Phys. Rev. Lett. 102, 173601 (2009).
 Pfeifer, M. & Fischer, P. Weak value amplified optical activity measurements. Opt. Express 19, 16508–16517 (2011).
 Shomroni, I., Bechler, O., Rosenblum, S. & Dayan, B. Demonstration of weak measurement based on atomic spontaneous emission. Phys. Rev. Lett. 111, 023604 (2013).
 Jayaswal, G., Mistura, G. & Merano, M. Observation of the Imbert–Fedorov effect via weak value amplification. Opt. Lett. 39, 2266–2269 (2014).
 Magaña Loaiza, O. S., Mirhosseini, M., Rodenburg, B. & Boyd, R. W. Amplification of angular rotations using weak measurements. Phys. Rev. Lett. 112, 200401 (2014).
 SalazarSerrano, L. J., Janner, D., Brunner, N., Pruneri, V. & Torres, J. P. Measurement of subpulsewidth temporal delays via spectral interference induced by weak value amplification. Phys. Rev. A 89, 012126 (2014).
 Tanaka, S. & Yamamoto, N. Information amplification via postselection: a parameterestimation perspective. Phys. Rev. A 88, 042116 (2013).
 Ferrie, C. & Combes, J. Weak value amplification is suboptimal for estimation and detection. Phys. Rev. Lett. 112, 040406 (2014).
 Jordan, A. N., MartínezRincón, J. & Howell, J. C. Technical advantages for weakvalue amplification: when less is more. Phys. Rev. X 4, 011031 (2014).
 Combes, J., Ferrie, C., Jiang, Z. & Caves, C. M. Quantum limits on postselected, probabilistic quantum metrology. Phys. Rev. A 89, 052117 (2014).
 Viza, G. I., MartínezRincón, J., Alves, G. B., Jordan, A. N. & Howell, J. C. Experimentally quantifying the advantages of weakvaluebased metrology. Phys. Rev. A 92, 032127 (2015).
 Ferrie, C. & Combes, J. How the result of a single coin toss can turn out to be 100 heads. Phys. Rev. Lett. 113, 120404 (2014).
 Feizpour, A., Xing, X. & Steinberg, A. M. Amplifying singlephoton nonlinearity using weak measurements. Phys. Rev. Lett. 107, 133603 (2011).
 Goggin, M. E. et al. Violation of the Leggett–Garg inequality with weak measurements of photons. Proc. Natl Acad. Sci. USA 108, 1256–1261 (2011).
 Groen, J. P. et al. Partialmeasurement backaction and nonclassical weak values in a superconducting circuit. Phys. Rev. Lett. 111, 090506 (2013).
 Feizpour, A., Hallaji, M., Dmochowski, G. & Steinberg, A. M. Observation of the nonlinear phase shift due to single postselected photons. Nat. Phys. 11, 905–909 (2015).
 Dmochowski, G. et al. Experimental demonstration of the effectiveness of electromagnetically induced transparency for enhancing crossphase modulation in the shortpulse regime. Phys. Rev. Lett. 116, 173002 (2016).
Acknowledgements
This work was funded by NSERC, CIFAR, Northrop Grumman Aerospace Systems NG Next, and the Fetzer Franklin Fund of the John E. Fetzer Memorial Trust. We would like to acknowledge A. Stummer’s design and construction of several electronic devices which were essential to this experiment.
Author information
Affiliations

Centre for Quantum Information and Quantum Control and Institute for Optical Sciences, Department of Physics, University of Toronto, 60 St George Street, Toronto, Ontario M5S 1A7, Canada
 Matin Hallaji,
 Amir Feizpour,
 Greg Dmochowski,
 Josiah Sinclair &
 Aephraim M. Steinberg

Canadian Institute For Advanced Research, 180 Dundas Street W., Toronto, Ontario M5G 1Z8, Canada
 Aephraim M. Steinberg
Contributions
All authors contributed equally to the results, interpretation and presentation of this Letter.
Competing financial interests
The authors declare no competing financial interests.
Author details
Matin Hallaji
Search for this author in:
Amir Feizpour
Search for this author in:
Greg Dmochowski
Search for this author in:
Josiah Sinclair
Search for this author in:
Aephraim M. Steinberg
Search for this author in:
Supplementary information
PDF files
 Supplementary information (324 KB)
Supplementary information