The wave–particle dual nature of light and matter and the fact that the choice of measurement determines which one of these two seemingly incompatible behaviours we observe are examples of the counterintuitive features of quantum mechanics. They are illustrated by Wheeler’s famous ‘delayed-choice’ experiment1, recently demonstrated in a single-photon experiment2. Here, we use a single ultracold metastable helium atom in a Mach–Zehnder interferometer to create an atomic analogue of Wheeler’s original proposal. Our experiment confirms Bohr’s view that it does not make sense to ascribe the wave or particle behaviour to a massive particle before the measurement takes place1. This result is encouraging for current work towards entanglement and Bell’s theorem tests in macroscopic systems of massive particles3.
The question of whether light behaves like a particle or wave had a long and strongly contested history until the advent of quantum mechanics, where it was accepted that it could indeed exhibit either behaviour. Conversely, it was de Broglie’s hypothesis of matter waves4 that deviated from the preceding view of massive bodies exclusively as particles, which was confirmed by the electron diffraction experiments of Davisson and Germer5. Even more bizarrely, the way in which an experiment is performed seems to induce one of these behaviours to the exclusion of the other. The question of whether a single photon in an interferometer passes through either one arm (as a particle) or both simultaneously (as a wave) led to Wheeler devising his famous gedanken experiment, which supposed that the decision of whether to attempt to measure particle or wave behaviour is made after the photon enters the interferometer. By removing the second beamsplitter of the interferometer (Fig. 1a), which-way information is revealed6, which precludes an interference measurement, while inserting the beamsplitter destroys information about the path taken by the photon and re-establishes a wave interference dependent on the phase difference ϕ between the arms.
Although many experiments have shown particle–wave duality with photons7, including delayed-choice schemes8,9,10, delayed-choice quantum eraser experiments11 and entanglement swapping using delayed choice12, only recently has the complete scheme proposed by Wheeler been realized experimentally 2. By simultaneously ensuring that only a single photon is present in the interferometer at once, and that the decision of interferometer configuration is relativistically separated from the photon’s entry to the interferometer, it was unambiguously shown that Wheeler’s supposition that such a choice affects the ‘past history’ of the photon was correct.
Recent advances in the trapping and cooling of atoms has led to the ability to readily observe wavelike phenomena with particles that have mass, such as the interference between two Bose–Einstein condensates13. However, progress towards demonstrating Wheeler’s experiment with massive particles, such as a delayed-choice Stern–Gerlach interferometer with metastable hydrogen14 or a spin interferometer with neutrons15, have been limited. Importantly, these experiments used beams containing more than one particle in the apparatus at any one time, rendering a meaningful test of Wheeler’s ideas impossible, at least at the quantum level. Nonetheless, they demonstrate an advantage of using massive particles over photons, the relatively slow velocity (compared to light) of the atoms through the interferometer allows an increased time for making the delayed choice.
Here, we report the first realization of Wheelers famous delayed-choice gedanken experiment with single massive particles. The only successful demonstration of Wheeler’s ideas so far has been achieved with single photons2. Here we use atoms, which is an important distinction, since atoms have many internal degrees of freedom. This allows coupling to the external environment through, for example, the atom’s sensitivity to magnetic and electric fields. Moreover, an atom has significant mass, which allows strong coupling to gravitational fields. These interactions of the atom with its environment are required for the appearance of decoherence; thus, in this sense an atom can be thought of as a more classical particle than a photon. As such, our experiment tests Wheeler’s ideas in a regime in which it has never been tested.
We use an ultracold (<1 nK) source of single atoms16 to implement Wheeler’s idea: that the behaviour of the atom can indeed be induced by our choice of measurement. Our experimental set-up closely mirrors that of the Mach–Zehnder scheme originally proposed by Wheeler (Fig. 1b), where essentially the roles of light and matter have been reversed. Atoms are released from an optical dipole trap (see Methods) and fall under gravity towards a delay-line detector (DLD) capable of imaging single He∗ atoms with three-dimensional information.
About 1 ms after releasing the atoms from the trap, a pair of laser beams are used to Bragg scatter the atoms into different momentum modes (see Methods)17, where for a Rabi frequency Ω, a Bragg pulse of duration tπ = π/Ω coherently transfers from one momentum mode to another in a two-state system18, and a pulse duration tπ/2 = π/(2Ω) transfers one momentum mode into an equal superposition of the two modes. The action of a π pulse is thus analogous to a mirror, while the π/2 pulse acts as a 50:50 beamsplitter. An arbitrary phase can be applied to the atomic wavefunction by controlling the phase of the Bragg pulses. In particular, we set the phase to zero for all pulses except for the first π/2 pulse, which carries an adjustable relative phase ϕ.
After applying the π pulse, a quantum random bit generator (see Methods) is triggered to decide whether the second π/2 pulse should be initiated, which is equivalent to the addition or removal of the second beamsplitter in the optical case (Fig. 1a). In our experiment, we use Bragg pulses of order 20 μs (and a π/2–π–π/2 sequence of 200 μs duration) and generate the random bit and implement its result 170 μs after the first beamsplitting pulse—thus ensuring that the choice of detection is made well after the atom passes the first beamsplitter and also that the atom has no prior knowledge about the final configuration of the interferometer.
If the second π/2 pulse is applied, then the arms of the interferometer are mixed, and the relative phase between the arms ϕ, generated at the first beamsplitter, can affect the probability of each atom being in a given momentum mode. Should this pulse be disabled, then there is a 50% chance that the atom will travel down either path of the interferometer in the ‘open’ configuration, which means that the average count rate for each momentum mode will be 50% irrespective of the phase ϕ applied. Instead of having a separate detector to measure counts in each arm of the interferometer, we can easily resolve the two momentum modes due to their arrival at different spatial positions and times on the same DLD (ref. 19; see Fig. 2).
It is interesting to contrast the photon demonstration of Wheeler’s experiment2 with the atomic one performed here. In the photon case the timing of the experiment is such that the small temporal width of the single-photon source (45 ns), combined with a large interferometer (48 m), allow the choice event to be space-like separated from the event where the photon reaches the first beamsplitter. In our experiment, the first beamsplitter is a light pulse which spatially overlaps the single-atom source, and thus the relevant temporal width for this operation is simply the duration of the π/2 pulse (20 μs). Thus space-like separation in our experiment is unfeasible; however, the slow velocity of the atom does allow a delayed choice in time, as implemented here.
As the data acquisition rates for a single-atom source are low (see Methods), we first demonstrate a delayed-choice interferometer with ∼1,000 atoms per experimental cycle in the inset of Fig. 3 (where we plot the normalized probability of finding atoms in the |0〉 state), where the result for each choice of ϕ is the average of 20 experimental cycles. The distinction between the removal (blue points) and application (red points) of the mixing π/2 pulse is very clear, as the former is ~50% irrespective of the phase ϕ, while the latter shows the expected sinusoidal dependence on ϕ, typical of a Mach–Zehnder interferometer.
This experimental procedure is then reproduced with a true single-atom source16, and compared to the large-number result. The result of this is shown in Fig. 3, where each experimental point is now the average of several thousand experimental cycles. It can be seen that the experimental points closely resemble that of Fig. 3 (inset), where fits to the experimental data give similar results to the large-number case. The main additional source of error for this data compared to the large-number version is shot noise due to limited counts. Also, the single-atom data are more susceptible to long-term drifts in the experiment, as data acquisition takes several weeks, as opposed to several hours for the large-number result.
We can quantify the single-atom nature of our source by analysing the statistics of atoms arriving at the output ports of the interferometer. To this end we calculate the second-order correlation function for the data shown in Fig. 3. We measure, see Fig. 4, a correlation function indicative of a strongly sub-Poissonian source, with a correlation parameter α (ref. 20) (equivalent to g2(0)) of α = 0.07 ± 0.03. The deviation we observe away from a perfect single-atom source (α = 0) is readily explained via the measured dark count rate of our detector, with the probability of observing a real count and a dark count in the same run of the experiment, yielding a lower limit to α of 0.06. This equates to observing, out of the nearly 30,000 runs of the experiment, ten runs in which two counts are observed.
As in the optical case2 we require each detector (see Fig. 2) to be unambiguously correlated to the path the atom took through the interferometer. To test this assumption, we use the ‘which-way’ parameter I = (N1 − N2)/(N1 + N2) (refs 6, 21, 22), where N1 and N2 are the number of atoms measured at the output ports with the interferometer in the open configuration. We measure I = 0.97 ± 0.05 when the first beamsplitting pulse is absent—effectively allowing only one path through the interferometer. To check the other path we replace the first beamsplitting pulse with a mirror pulse, here we measure I = 0.95 ± 0.05, indicating that the ports of the interferometer allow excellent which-way information.
Further to this analysis, we can estimate the visibility when the interferometer is in the ‘open’ configuration by fitting a sinusoidal curve to the open data (blue squares in Fig. 3) and find a value of V = 0.03 ± 0.04. Consistent with theoretical predictions6,23, and demonstrated for the more general intermediate case with photons24, we expect the complementarity parameter for our interferometer to follow the inequality: V2 + D2 ≤ 1. For the open case we measure V2 + D2 = 0.92 ± 0.08, where D is the distinguishability, given by the average of the which-way parameters. In the absence of information loss, one expects the complementarity parameter to be unity; in our case, the deviation from unity is attributable to imperfections in the Bragg pulses which reduce our distinguishability. The ‘closed’ configuration could be investigated in an analogous way by implementing the final beamsplitter, as could the intermediate case in which the Bragg beamsplitter pulse reflectivity is varied.
Wheeler’s thought experiment is important since it tries to force a classical view of reality on to a quantum system. If one holds the view that to observe interference at the detector the photon must have traversed both arms (as a wave) of the interferometer (and conversely that the lack of interference unambiguously demonstrates the photon has traversed a single arm (as a particle)) then the ‘delayed’ choice creates a conundrum. In this picture, the choice of detection (delayed until after the photon has passed the first beamsplitter) is correlated with observing interference or no interference—and thus it seems that a future event (the method of detection) causes the photon to decide its past. If such a perspective seems untenable with a fast-moving massless photon, then our experiment, which uses a slow-moving massive helium atom (and thus is closer to our classical notions), makes this view of reality seem even more unlikely.
Source of ultracold He∗.
The experimental set-up is largely based on refs 25, 26. Ultracold 4He∗ is magnetically trapped and evaporatively cooled27 to just below the Bose–Einstein condensate transition temperature (∼1 μK). Approximately 104 atoms are transferred into a vertical optical dipole trap by ramping up the intensity of a far red-detuned focused laser beam in the direction of gravity over 200 ms. The magnetic trap is switched off and the only magnetic field present is generated by our magnetic field stabilization ‘nullerometer’28, which provides a bias magnetic field ∼1 Gauss. Then, the dipole trap is ramped down over 100 ms, resulting in a trap with harmonic frequencies of (ωx, ωy, ωz)/2π = (1800,1800,12) Hz. The trap depth (equivalent to a temperature of a few nanokelvin) is then held at this point for two seconds, which allows the majority of the thermal atoms to exit the trap.
To obtain a single-atom source16, we induce Penning ionization losses in the cloud described above by spin flipping the atoms from the mj = 1 state to the mj = 0 state with radio frequency (RF) radiation, which increases the rate of two-body Penning ionization loss by ∼5 orders of magnitude29. The two-body collisional lifetime of mj = 0 atoms in our dipole trap is (∼10 ms), which is much shorter than the lifetime of mj = 1 atoms in the same trap (∼25 s) or the radiative lifetime of the metastable helium excited state (7,870 s; ref. 30). By holding the mj = 0 atoms for 5 s we obtain a single atom in 50% of experimental cycles, and no atoms otherwise, depending on whether we start with an odd or even number of atoms in the trap, respectively. As each experimental cycle represents obtaining a single atom (or lack thereof), we are able to determine with confidence (with reference to detector efficiency ∼20% and trap lifetime) that we have only at most a single atom present16. The atom is then released from the trap by switching off the dipole trapping beam.
The Bragg beams are applied ∼1 ms after the atoms are released from the dipole trap and have a detuning ∼280 GHz to the red of the 21S0–23P2 transition, and a relative detuning of 47 kHz between the beams. The interferometer uses a π/2–π–π/2 pulse sequence, with each pulse being 20 μs in duration and the π pulse having ∼1.5 times the intensity. The time between the beamsplitting pulses and the mirror pulse is ∼100 μs and a Quantis OEM quantum random bit generator (1D Quantique, model number: Quantis, P/N:0600684A210) is triggered and the resulting ‘on’ or ‘off’ state is latched to an RF switch to randomly determine whether the second beamsplitting pulse is applied 70 μs after the mirror pulse finishes, which provides the ‘delayed choice’ for the experiment.
A.G.T. acknowledges the support of the Australian Research Council through the Future Fellowship grant FT100100468. The authors would like to acknowledge the technical assistance of C. Dedman as well as C. Savage for informative discussions.