**Appendix 2.F Supplementary Tables**

**3.2 Methods**

**3.2.1 On Averaging, Reynolds Decomposition and Taylor’s Hypothesis 70**

Most methods used to retrieve the dissipation rate require spatially resolved velocity statistics although the velocity is recorded only at a single point and as a function of time in many experiments. Therefore, prior to estimating the energy dissipation rate, the one-dimensional velocity time-record should be first mapped onto a spatially resolved velocity field. This is achieved by invoking Taylor’s hypothesis, which requires a Reynolds decomposition of the velocity time-record by separating the velocity fluctu- ations from the mean velocity. To perform the Reynolds decomposition, we first have to clarify what is meant by the mean velocity.

Generally, we have to distinguish between the global mean velocity* U* = ⟨

*(*

**u***)⟩=*

**x**, t*U*1, which is independent of time and space since

**e***(*

**u***) is assumed to be statistically stationary and homogeneous, the volume-averaged velocity ⟨*

**x**, t*(*

**u***)⟩*

**x**, t^{R}over a sphere of radius

*R*, the time-averaged velocity⟨

*(*

**u***)⟩*

**x**, t*τ*over a time interval

*τ*, and the ensemble- averaged velocity ⟨

*(*

**u***)⟩*

**x**, t^{N}over

*N*realizations [5, 41, among others]. In this work,

⟨·⟩denotes the global mean, i.e. for infinitely large averaging windows in time or space.

Implicitly, ⟨* u*(

*)⟩*

**x**, t^{R}= 3

*/*(4

*πR*

^{3})

^{RRR}

_{0}

^{R}d

*(*

**x**u*) and ⟨*

**x**, t*(*

**u***)⟩*

**x**, t^{τ}=

^{1}

_{τ}

^{R}

_{−τ /2}

^{τ /2}d

*t*

^{′}

*(*

**u**

**x**, t^{′}) are, respectively, local volume and time averages as both

*R*and

*τ*are typically

finite. In the limit of *R, τ* → ∞, ⟨* u*(

*)⟩*

**x**, t*R*and ⟨

*(*

**u***)⟩*

**x**, t*τ*tend to

*U⃗*. For repeatable experiments where identical experimental conditions are guaranteed, ⟨

*(*

**u***)⟩*

**x**, t^{N}tends to

*when*

**U***N*→ ∞.

Here we define the mean of a one-dimensional velocity time-record in the longitudinal direction by

*U**τ* =⟨*u*1(*t*)⟩*τ* = 1
*τ*

Z *τ /*2

−*τ /*2d*t*^{′}*u*1(*t*^{′})*,* (3.1)

such that *U* = lim*τ*→∞*U**τ* where *τ* is the *averaging window*. It should be noted that
the global mean of the transverse velocity will be equal to zero, i.e. ⟨*u*2*,*3(*t*)⟩^{τ} = 0 when
*τ* → ∞, since here it is assumed that they are orthogonal to the mean flow direction.

According to the Reynolds decomposition, the longitudinal velocity time record
is composed of the mean velocity *U* and the random velocity fluctuation component
*u*^{′}_{1}(*t*) =*u*1(*t*)−*U* so that the mean of the longitudinal velocity fluctuations⟨*u*^{′}_{1}(*t*)⟩= 0.

This is also true for other components of the velocity.

In certain circumstances, it is possible to map*u*^{′}_{1}(*t*) from time to space coordinates
by applying the Taylor’s (frozen-eddy) hypothesis [41, 156], which relates temporal
and spatial velocity statistics. Taylor argues that eddies can be regarded as *frozen*
in time if they are passing the probing volume much faster than they evolve in time.

This is the case if the turbulence intensity *I* =*σ**u*^{′}_{1}*/U* is much smaller than the unity,
i.e. *I* ≪1, where*σ**u*^{′}_{1} =⟨*u*^{′2}_{1}⟩^{1/2} is the Root-Mean-Square (RMS) velocity fluctuation.

Then, the series of time lags ∆*t*=*t*−*t*0 relative to the start time *t*0 is mapped onto a
distance vector with * x*=

*0+*

**x***U*∆

*t*1 [156] where

**e***0 is the initial position at time*

**x***t*0. This approach is found to be reliable for

*I*≲0

*.*25 [54, 157, 158] while it has been shown to fail when

*I >*0

*.*5 [159]. The application of Taylor’s hypothesis is inaccurate in case of large-scale variations of the velocity fluctuation field comparable to the mean velocity, which are known as “random sweeping velocity” [160, 161] and which can be approximated by the turbulence intensity [158]. Complicating the estimation of the mean velocity, random sweeping causes the mean energy dissipation rate to be consistently overestimated [137, 162].

One way to cope with non-stationary velocity time records is to evaluate the mean
velocity for a subset of this signal. If the averaging time *τ* is finite, the time average*U**τ*

may differ from the mean velocity *U* causing a systematic bias in the subsequent data
analysis. The estimation variance of the time average *U**τ* can be analytically expressed
as [5, 41, among others]

⟨(*U**τ* −*U*)^{2}⟩ ≈ 2⟨*u*^{′2}_{1}⟩*T*

*τ* *,* (3.2)

where *T* is the integral time scale and ⟨*u*^{′2}_{1}⟩ the variance of the velocity time series.

Notably, the size of the averaging window has to be large enough such that it fulfills

⟨*u*^{′}_{1}(*t*)⟩*τ* ≈0 to apply the Reynolds decomposition. This expression can be converted
to space invoking Taylor’s hypothesis.

**3.2.2** **Preliminaries on Second-Order Statistics**

As discussed in detail below, the mean energy dissipation rate can be related to second- order statistics of the velocity field, either in terms of velocity gradients or in terms of velocity increments. In any case, the two-point velocity covariance tensor turns out to be the central quantity of interest, from which the second-order structure function tensor, the spectral energy tensor and the velocity gradient covariance tensor can be obtained.

In the following, we assume zero-mean SHI turbulence so that two-point quantities
depend only on the separation vector* r*, all averages are invariant under rotations of
the coordinate system, and the mean squared velocity fluctuation is identical for all
velocity components, i.e. ⟨

*u*

^{′2}⟩ = ⟨

*u*

^{′2}

_{1}⟩ = ⟨

*u*

^{′2}

_{2}⟩ = ⟨

*u*

^{′2}

_{3}⟩. We provide an overview of the most relevant definitions, their notation and conventions. This section does not explicitly discuss the effect of the averaging window, but the definitions presented can be applied to windowed inputs with no or straightforward modifications.

Under the given assumptions, the two-point velocity covariance tensor takes the form [e.g. 5, 45, 46]

*R**ij*(* r*) = ⟨

*u*

^{′}

_{i}(

*+*

**x***)*

**r**, t*u*

^{′}

_{j}(

*)⟩=⟨*

**x**, t*u*

^{′2}⟩

*g*(*r*)*δ**ij* + [*f*(*r*)−*g*(*r*)]*r**i**r**j*

*r*^{2}

*,* (3.3)

where *f*(*r*) = *R*11(*r*)*/R*11(0) and *g*(*r*) = *f*(*r*) +*r∂**r**f*(*r*)*/*2 are the longitudinal and
transverse autocorrelation functions, respectively, with *f*(0) =*g*(0) = 1. Notably, if
one chooses * r* =

*r*1,

**e***R*11(

*r*) = ⟨

*u*

^{′2}⟩

*f*(

*r*),

*R*22(

*r*) =

*R*33(

*r*) = ⟨

*u*

^{′2}⟩

*g*(

*r*), and all other components vanish [e.g. 5]. As a remarkable consequence,

*R*

*ij*(

*) is uniquely defined by*

**r***f*(

*r*) in isotropic turbulence. As mentioned below, the integral length scale as well as the Taylor microscale are determined by

*f*(

*r*) [5].

Analogously, a covariance tensor can be defined for velocity increments, i.e. the second-order velocity structure function tensor [5, 42]

*D**ij*(* r*) =⟨[

*u*

^{′}

_{i}(

*+*

**x***)−*

**r**, t*u*

^{′}

_{i}(

*)]*

**x**, t^{h}

*u*

^{′}

_{j}(

*+*

**x***)−*

**r**, t*u*

^{′}

_{j}(

*)*

**x**, t^{i}⟩ (3.4)

=*D**N N*(*r*)*δ**ij* + [*D**LL*(*r*)−*D**N N*(*r*)]*r**i**r**j*

*r*^{2} *.* (3.5)

The longitudinal second-order structure function *D*11(*r*) is related to *f*(*r*) by [e.g.

5, 42]

*D*11(* r* =

*r*1) =

**e***D*

*LL*(

*r*) = ⟨(

*u*

^{′}

_{1}(

*+*

**x***r*1

**e***, t*)−

*u*

^{′}

_{1}(

*))*

**x**, t^{2}⟩= 2⟨

*u*

^{′2}⟩(1−

*f*(

*r*))

*.*(3.6) As explained below, measuring the longitudinal second-order structure function

*D*

*LL*(

*r*), the mean energy dissipation rate can be inferred from the inertial-range scaling of the longitudinal structure function (cf. Eq. (3.15)).

Furthermore, the velocity gradient covariance tensor can also be defined in terms

of the velocity covariance tensor
*R**ijkl*(* r*) =

**∂u*^{′}_{i}(* x, t*)

*∂x**k*

*∂u*^{′}_{j}(* x, t*)

*∂x**l*

+

=−lim

*r*→0*∂**r**k**∂**r**l**R**ij*(* r*)

*.*(3.7) Since the local and instantaneous energy dissipation rate (cf. Eq. (3.11)) is defined in terms of the strain rate tensor

*S*

*ik*= (

*∂u*

^{′}

_{i}(

*)*

**x**, t*/∂x*

*k*+

*∂u*

^{′}

_{k}(

*)*

**x**, t*/∂x*

*i*)

*/*2, the mean energy dissipation rate can be directly related to contractions of the velocity gradient covariance tensor. Note that in a turbulent flow with zero-mean velocity, the strain rate tensor

*S*

*ik*equals the fluctuation strain rate tensor

*s*

*ik*.

The two-point velocity covariance tensor can be expressed in Fourier space through the spectral energy tensor [5]

Φ*ij*(* κ*) = 1
(2

*π*)

^{3}

Z Z Z +∞

−∞ *R**ij*(* r*)

*e*

^{−iκ·r}d

*(3.8)*

**r**,where* κ* is the wave vector. For SHI turbulence, Φ

*ij*(

*) takes the form Φ*

**κ***ij*(

*) =*

**κ***E*(

*κ*)

4*πκ*^{2}

*δ**ij* − *κ**i**κ**j*

*κ*^{2}

(3.9)

where*E*(*κ*) is the energy spectrum function.

Since access to the full energy spectrum function is not always available, one- dimensional spectra are of interest, too. The mean energy dissipation rate can be estimated from the inertial range scaling of the longitudinal one-dimensional spectrum (as shown in Eq. (3.17)), which can be calculated by both the energy spectrum function

and the velocity covariance tensor [5]

*E*11(*κ*1) = ^{Z} ^{∞}

*κ*1

*E*(*κ*)

*κ* 1− *κ*^{2}_{1}
*κ*^{2}

!

d*κ*= 1
*π*

Z ∞

−∞*R*11(* e*1

*r*1)

*e*

^{−iκ}

^{1}

^{r}

^{1}d

*r*1

*,*(3.10) with the wavenumber

*κ*1 corresponding to the

*1-direction and*

**e***R*11(0) = ⟨

*u*

^{′2}⟩ =

R∞

0 *E*11(*κ*1)d*κ*1.

This concludes the second-order statistics in terms of the velocity that we consider in the following to determine the mean energy dissipation rate.