Experiments Einstein could only dream of


Editor's Introduction

Measurement of the instantaneous velocity of a Brownian particle

annotated by

Sometimes, scientists have to wait for technology to catch up.  While working on Brownian motion, Albert Einstein proposed ideas that he did not yet have the tools to examine, prompting him to conclude that the instantaneous velocity of a Brownian particle would be impossible to measure in practice.  Now, almost 100 years later, scientists have the technology to measure the instantaneous velocity of a Brownian particle, proving Einstein wrong in the process.     

Paper Details

Original title
Measurement of the instantaneous velocity of a Brownian particle
Mark Raizen
Original publication date
Science 25 June 2010: Vol. 328 no. 5986 pp. 1673-1675
Issue name


Brownian motion of particles affects many branches of science. We report on the Brownian motion of micrometer-sized beads of glass held in air by an optical tweezer, over a wide range of pressures, and we measured the instantaneous velocity of a Brownian particle. Our results provide direct verification of the energy equipartition theorem for a Brownian particle. For short times, the ballistic regime of Brownian motion was observed, in contrast to the usual diffusive regime. We discuss the applications of these methods toward cooling the center-of-mass motion of a bead in vacuum to the quantum ground motional state.


In 1907, Albert Einstein published a paper in which he considered the instantaneous velocity of a Brownian particle (12). By measuring this quantity, one could prove that “the kinetic energy of the motion of the centre of gravity of a particle is independent of the size and nature of the particle and independent of the nature of its environment.” This is one of the basic tenets of statistical mechanics, known as the equipartition theorem. However, because of the very rapid randomization of the motion, Einstein concluded that the instantaneous velocity of a Brownian particle would be impossible to measure in practice.

We report here on the meastaurement of the instantaneous velocity of a Brownian particle in a system consisting of a single, micrometer-sized SiO2 bead held in a dual-beam optical tweezer in air, over a wide range of pressures. The velocity data were used to verify the Maxwell-Boltzmann velocity distribution and the equipartition theorem for a Brownian particle. The ability to measure instantaneous velocity enables new fundamental tests of statistical mechanics of Brownian particles and is also a necessary step toward the cooling of a particle to the quantum ground motional state in vacuum.

The earliest quantitative studies of Brownian motion were focused on measuring velocities, and they generated enormous controversy (3, 4). The measured velocities of Brownian particles (3) were almost 1000-fold smaller than what was predicted by the energy equipartition theoremRecent experiments with fast detectors that studied Brownian motion in liquid (5–7) and gaseous (8–10) environments observed nondiffusive motionof a Brownian particle.

Einstein’s theory predicts that [Δx(t)]2 =2Dt, where [Δx(t)]2 is the mean square displacement (MSD) in one dimension of a free Brownian particle during time t, and D is the diffusion constant (11). The diffusion constant can be calculated by D=kBT/γ, where kB is Boltzmann’s constantT is the temperature, and γ is the Stokes friction coefficient.The mean velocity measured over an interval of time v¯ [ Δx(t) ]2 /t=2D/t. This diverges as t approaches 0 and therefore does not represent the real velocity of the particle (12).

The equation [Δx(t)]2 =2Dt, however, is valid only when t>>τp; that is, in the diffusive regime. Here, τp=m/γ is the momentum relaxation time of a particle with mass m. At very short time scales (t<<τp), the dynamics of a particle are dominated by its inertia, and the motion is ballistic. The dynamics of a Brownian particle over all time scales can be described by a Langevin equation (12). The MSD of a Brownian particle at very short time scales is predicted to be [Δx(t)]2 =(kBT/m)t2, and its instantaneous velocity can be measured as v=Δx(t)/t, when t<<τp(13).

For a 1-μm-diameter silica (SiO2) sphere in water, τp is about 0.1 μs and the root mean square (rms) velocity is about 2 mm/s in one dimension. To measure the instantaneous velocity with 10% uncertainty, one would require 2-pm spatial resolution in 10 ns, far beyond what is experimentally achievable today (7). Because of the lower viscosity of gas, compared with liquid, the τp of a particle in air is much larger. This lowers the technical demand for both temporal and spatial resolution. The main difficulty of performing high-precision measurements of a Brownian particle in air, however, is that the particle will fall under the influence of gravity. We overcome this problem by using optical tweezers to simultaneously trap and monitor a silica bead in air and vacuum, allowing long-duration, ultra–high-resolution measurements of its motion. This technology was unavailable and even considered impossible during Einstein's time.

We overcome this problem by using optical tweezers to simultaneously trap and monitor a silica bead in air and vacuum, allowing long-duration, ultra–high-resolution measurements of its motion.

For small displacements, the effect of optical tweezers on the bead’s motion can be approximated by a harmonic potential. The MSD of a Brownian particle in an underdamped harmonic trap in air can be obtained by solving the Langevin equation (14)

[Δx(t)]2 =2kBTmω02[ 1et/2τp(cosω1t+sinω1t2ω1τp) ]
































where ω0 is the resonant frequency of the trap and ω1ω021/(2τp)2.
































The normalized velocity autocorrelation function (VACF) of the particle is (14)
































































In the simplified scheme of our optical trap and vacuum chamber (Fig. 1), the trap is formed inside a vacuum chamber by two counterpropagating laser beams focused to the same point by two identical aspheric lenses with focal lengths of 3.1 mm and numerical apertures of 0.68 (15). The two 1064-nm-wavelength laser beams are orthogonally polarized, and their frequencies differ by 160 MHz to avoid interference. The scattering forces exerted on the bead by the two beams cancel, and the gradient forces near the center of the focus create a three-dimensional harmonic potential for the bead. When the bead deviates from the center of the trap, it deflects both trapping beams. The position of the bead is monitored by measuring the deflection of one of the beams, which is split by a mirror with a sharp edge. The difference between the two halves is measured by a fast balanced detector (716).
































figure 1.jpg

Fig. 1.  Simplified schematic showing the counterpropagating dual-beam optical tweezers, and a novel detection system that has a 75-MHz bandwidth and ultralow noise. The s-polarized beam is reflected by a polarizing beam-splitter cube after it passes through a trapped bead inside a vacuum chamber. For detection, it is split by a mirror with a sharp edge. The p-polarized beam passes through the cube.

Figure 1

The authors present a simplified sketch of their optical trap. The arrows indicate the direction of the laser beams that are involved in the suspension of the Brownian particle. Only the s-polarized light travels to the detector, because of the arrangement of the optical circuit. The polarizing beam splitter cube only reflects the s-polarized light to that direction.

See the actual instrument used by the authors

These are pictures of the actual instruments the authors used to perform their experiments. This figure shows the optical setup as it looked when the experiemnts were conducted. The optical setup shown in this figure includes many optical components that were not used in these experiments. However, you can still get a feeling of the size of the optical setup from this more complex figure.

pic 13 optical trapping and cooling Jan 11, 2011.jpg

See a bead suspended in the optical trap.

This figure shows a bead trapped in the chamber.

trapped bead in vacuum.jpg
































The lifetime of a bead in our trap in air is much longer than our measurement times over a wide range of pressures and trap strengths.We have tested it by trapping a 4.7-μm bead in air continuously for 46 hours, during which the power of both laser beams was repeatedly changed from 5 mW to 2.0 W. The trap becomes less stable in vacuum. The lowest pressure at which we have trapped a bead without extra stabilization is about 0.1 Pa.
































For studying the Brownian motion of a trapped bead, unless otherwise stated, the powers of the two laser beams were 10.7 and 14.1 mW (15), the diameter of the bead was 3 μm, the temperature of the system was 297 K, and the air pressure was 99.8 or 2.75 kPa. The trapping was stable and the heating due to laser absorption was negligible under these conditions. In typical samples of position and velocity traces of a trapped bead (Fig. 2), the position traces of the bead at these two pressures appear to be very similar.On the other hand, the velocity traces are clearly different. The instantaneous velocity of the bead at 99.8 kPa changes more frequently than that at 2.75 kPa, because the momentum relaxation time is shorter at higher pressure.

































Fig. 2. One-dimensional trajectories of a 3-μm-diameter silica bead trapped in air at 99.8 kPa (A) and 2.75 kPa (B). The instantaneous velocities of the bead corresponding to these trajectories are shown in (C) and (D).

Panels A and B

In this figure, the authors show the specificity of their optical trap. Remember, the goal of this experiment is to measure the velocity of the trapped Brownian particle. Panels A and B show the particle, at different pressures, remaining somewhat random while being held in the optical trap.

Panels C and D

Panels C and D match up with Panels A and B and show that while the Brownian particle is being held somewhat random in the optical trap, the authors are still able to measure the velocity of the particle's motion.
































Figure 3 shows the MSDs of a 3-μm silica bead as a function of time. The measured MSDs fit with Eq. 1 over three decades of time for both pressures. The calibration factor α = position/voltage of the detection system is the only fitting parameter of Eq. 1 for each pressure. τp and ω0 are obtained from the measured normalized VACF. The two values of α obtained for these two pressures differ by 10.8%. This is because the vacuum chamber is distorted slightly when the pressure is decreased from 99.8 to 2.75 kPa. The measured MSDs are completely different from those predicted by Einstein’s theory of Brownian motion in a diffusive regime The slopes of measured MSD curves at short time scales are double those of the MSD curves of diffusive Brownian motion in the log-log plot (Fig. 3A). This is because the MSD is proportional to t2 for ballistic Brownian motion, whereas it is proportional to t for diffusive Brownian motion. In addition, the MSD curves are independent of air pressure at short time scales, which is predicted by [Δx(t)]2 =(kBT/m)t2 for ballistic Brownian motion, whereas the MSD in the diffusive regime does depend on the air pressure. At long time scales, the MSD saturates at a constant value because of the optical trap. Figure 3B displays more detail of the Brownian motion at short time scales. It clearly demonstrates that we have observed ballistic Brownian motion.

































Fig. 3.  (A) The MSDs of a 3-μm silica bead trapped in air at 99.8 kPa (red square) and 2.75 kPa (black circle). They are calculated from 40 million position measurements for each pressure. The “noise” signal (blue triangle) is recorded when there is no particle in the optical trap. The solid lines are theoretical predictions of Eq. 1. The prediction of Einstein’s theory of free Brownian motion in the diffusive regime is shown in dashed lines for comparison. (B) MSDs at short time scales are shown in detail. The dash-dotted line indicates ballistic Brownian motion of a free particle.

Panel A

The first thing to notice on these two graphs is their different scales. In panel A, the authors are testing the hypothesis that Brownian motion is composed only of diffusive motion. However, their measurements do not line up with what diffusive motion of this particle should look like. (The diffusive motion equation is shown in the upper left-hand corner. The authors used this equation to plot the dashed lines - the predicted diffusive motion for a particle of this size.)

The 'noise' graph, shown here as triangles, are the MSD recordings when a particle is not in the optical trap.  You can see that these values are just about zero, indicating that the optical trap itself is not contributing to the MSD measurements of a Brownian particle at short time scales.  

Panel B

Here, the authors use the equation for ballistic motion, which you can see corresponds with their measurements.  

For both graphs, you can see that pressure does not affect the MSD measurements of a Brownian particle.  
































The distributions of the measured instantaneous velocities (Fig. 4A) agree very well with the Maxwell-Boltzmann distribution. The measured rms velocities are vrms = 0.422 mm/s at 99.8 kPa and vrms = 0.425 mm/s at 2.75 kPa. These values are very close to the prediction of the energy equipartition theorem, vrms=kBT/m, which is 0.429 mm/s. As expected, the velocity distribution is independent of pressure. The rms value of the noise signal is 0.021 mm/s, which means we have 1.0 Å spatial resolution in 5 μs. This measurement noise is about 4.8% of the rms velocity. Figure 4A represents direct verification of the Maxwell-Boltzmann distribution of velocities and the equipartition theorem of energy for Brownian motion. For a Brownian particle in liquid, the inertial effects of the liquid become important. The measured rms velocity of the particle will be vrms=kBT/min the ballistic regime, where the effective mass m* is the sum of the mass of the particle and half of the mass of the displaced fluid (17). This is different from the equipartition theorem. To measure the true instantaneous velocity in liquid as predicted by the equipartition theorem, the temporal resolution must be much shorter than the time scale of acoustic damping, which is about 1 ns for a 1-μm particle in liquid (17).

































Fig. 4. (A) The distribution of the measured instantaneous velocities of a 3-μm silica bead. The statistics at each pressure is calculated from 4 million instantaneous velocities. The solid lines are Maxwell-Boltzmann distributions. We obtained vrms = 0.422 mm/s at 99.8 kPa (red square) and vrms = 0.425 mm/s at 2.75 kPa (black circle) from the measurements. The rms value of the noise (blue triangle) is 0.021 mm/s. (B) The normalized velocity autocorrelation functions of the 3-μm bead at two different pressures. The solid lines are fittings with Eq. 2.

Panel A

Here, the authors compare the properties of their Brownian particle in the optical trap to known theories of how that particle should be behaving (specifically, the Maxwell-Boltzmann velocity distribution). As you can see here, the authors' experimental measurements align with the predicted measurements, indicating that the Brownian particle is behaving as it should, and the results shown in Fig. 3 are not the result of the Brownian particle acting strangely.

Panel B

The velocity autocorrelation function (VCAF) is calculated during analysis of the diffusive properties of a particle. If the motion of the particle follows an oscillatory pattern, the VCAF will characterize the oscillations because the velocity of the atoms will self-correlate in a periodic fashion. 

In this figure, the authors normalize the VCAF, and from there are able to find (Tau p), the momentum relaxation time, and wo, the resonant frequency of the trap.  
































Figure 4B shows the normalized VACF of the bead at two different pressures. At 2.75 kPa, one can see the oscillations due to the optical trap. Equation 2 is independent of the calibration factor α of the detection system. The only independent variable is time t, which we can measure with high precision. Thus the normalized VACF provides an accurate method to measure τp ω0. By fitting the normalized VACF with Eq. 2, we obtained τp = 48.5 ± 0.1 μs, ω0 = 2π · (3064 ± 4) Hz at 99.8 kPa and τp = 147.3 ± 0.1 μs, ω0 = 2π · (3168 ± 0.5) Hz at 2.75 kPa. The trapping frequency changed by 3% because of the distortion of the vacuum chamber at different pressures. For a particle at a certain pressure and temperature, τp should be independent of the trapping frequency. We verified this by changing the total power of the two laser beams from 25 to 220 mW The measured τp changed less than 1.3% for both pressures, thus proving that the fitting method is accurate, and the heating due to the laser beams (which would change the viscosity and affect τp) is negligible. We can also calculate the diameter of the silica bead from the τp value at 99.8 kPa (18). The obtained diameter is 2.79 μm. This is within the uncertainty range given by the supplier of the 3.0-μm silica beads. We used this value in the calculation of MSD and normalized VACF.
































The ability to measure the instantaneous velocity of a Brownian particle will be invaluable in studying nonequilibrium statistical mechanics (1920) and can be used to cool Brownian motion by applying a feedback force with a direction opposite to the velocity (2122). In a vacuum, our optically trapped particle should be an ideal system for investigating quantum effects in a mechanical system (162325) because of its near-perfect isolation from the thermal environment. Combining feedback cooling and cavity cooling, we expect to cool the Brownian motion of a bead starting from room temperature to the quantum regime, as predicted by recent theoretical calculations (2425). We have directly verified the energy equipartition theorem of Brownian motion. However, we also expect to observe deviation from this theorem when the bead is cooled to the quantum regime. The kinetic energy of the bead will not approach zero even at 0 K because of its zero-point energy. The rotational energy of the bead should also become quantized.
































References and Notes
































  1. Einstein, Theoretische Bemerkungen über die Brownsche Bewegung. Zeit. f. Elektrochemie 13, 41 (1907).

  2. Einstein, Investigations on the Theory of the Brownian Movement, R. Fürth, Ed., A. D. Cowper, Transl. (Methuen, London, 1926), pp. 63–67.

  3. F. M. Exner, Notiz zu Brown’s Molecularbewegung. Ann. Phys. 2, 843 (1900).

  4. M. Kerker, Brownian movement and molecular reality prior to 1900. J. Chem. Educ. 51, 764 (1974).

  5. B. Lukic et al., Direct observation of nondiffusive motion of a Brownian particle. Phys. Rev. Lett. 95, 160601 (2005).

  6. Y. Han et al., Brownian motion of an ellipsoid. Science 314, 626 (2006).

  7. I. Chavez, R. Huang, K. Henderson, E.-L. Florin, M. G. Raizen, Development of a fast position-sensitive laser beam detector. Rev. Sci. Instrum. 79, 105104 (2008).

  8. P. D. Fedele, Y. W. Kim, Direct measurement of the velocity autocorrelation function for a Brownian test particle. Phys. Rev. Lett. 44, 691 (1980).

  9. J. Blum et al., Measurement of the translational and rotational Brownian motion of individual particles in a rarefied gas. Phys. Rev. Lett. 97, 230601 (2006).

  10. R. Burnham, P. J. Reece, D. McGloin, Brownian dynamics of optically trapped liquid aerosols. In press; preprint available at http://arxiv.org/abs/0907.4582.

  11. Einstein, Über die von der molekularkinetischen Theorie der Wärme geforderte Bewegung von in ruhenden Flüssigkeiten suspendierten Teilchen. Ann. Phys. 17, 549 (1905).

  12. P. Langevin, C. R. Acad. Sci. (Paris) 146, 530 (1908).

  13. G. E. Uhlenbeck, L. S. Ornstein, On the theory of the Brownian motion. Phys. Rev. 36, 823 (1930). CrossRef

  14. M. C. Wang, G. E. Uhlenbeck, On the theory of the Brownian motion II. Rev. Mod. Phys. 17, 323 (1945).

  15. Materials and methods are available as supporting material on Science online.

  16. K. G. Libbrecht, E. D. Black, Toward quantum-limited position measurements using optically levitated microspheres. Phys. Lett. A 321, 99 (2004).

  17. R. Zwanzig, M. Bixon, Compressibility effects in the hydrodynamic theory of Brownian motion. J. Fluid Mech. 69, 21 (1975).

  18. A. Moshfegh, M. Shams, G. Ahmadi, R. Ebrahimi, A novel surface-slip correction for microparticles motion. Colloids Surf. A Physicochem. Eng. Asp. 345, 112 (2009).

  19. R. Kubo, Brownian motion and nonequilibrium statistical mechanics. Science 233, 330 (1986).

  20. G. M. Wang, E. M. Sevick, E. Mittag, D. J. Searles, D. J. Evans, Experimental demonstration of violations of the second law of thermodynamics for small systems and short time scales. Phys. Rev. Lett. 89, 050601 (2002).

  21. A. Hopkins, K. Jacobs, S. Habib, K. Schwab, Feedback cooling of a nanomechanical resonator. Phys. Rev. B 68, 235328 (2003).

  22. D. Kleckner, D. Bouwmeester, Sub-kelvin optical cooling of a micromechanical resonator. Nature 444, 75 (2006).

  23. Ashkin, J. M. Dziedzic, Optical levitation in high vacuum. Appl. Phys. Lett. 28, 333 (1976).

  24. D. E. Chang et al., Cavity opto-mechanics using an optically levitated nanosphere. Proc. Natl. Acad. Sci. U.S.A. 107, 1005 (2010).

  25. O. Romero-Isart, M. L. Juan, R. Quidant, J. Ignacio Cirac, Towards quantum superposition of living organisms. N. J. Phys. 12, 033015 (2010).

  26. M.G.R. acknowledges support from the Sid W. Richardson Foundation and the R. A. Welch Foundation grant number F-1258. D.M. acknowledges support from El Consejo Nacional de Ciencia y Tecnología (CONACYT) for his graduate fellowship (206429). The authors would also like to thank E.-L. Florin and Z. Yin for helpful discussions and I. Popov for his help with the experiment.